Top-Quark Physics at the LHC

# Top-Quark Physics at the LHC

Kevin Kröninger Technische Universität Dortmund, Fakultät Physik, Otto-Hahn-Str. 4, 44227 Dortmund, Germany
Deutsches Elektronen-Synchrotron (DESY), Notkestr. 85, 22607 Hamburg, Germany
Humboldt-Universität zu Berlin, Institut für Physik, Newtonstraße 15, 12489 Berlin, Germany
Andreas B. Meyer and Peter Uwer Technische Universität Dortmund, Fakultät Physik, Otto-Hahn-Str. 4, 44227 Dortmund, Germany
Deutsches Elektronen-Synchrotron (DESY), Notkestr. 85, 22607 Hamburg, Germany
Humboldt-Universität zu Berlin, Institut für Physik, Newtonstraße 15, 12489 Berlin, Germany
###### Abstract

The top quark is the heaviest of all known elementary particles. It was discovered in 1995 by the CDF and DØ experiments at the Tevatron. With the start of the LHC in 2009, an unprecedented wealth of measurements of the top quark’s production mechanisms and properties have been performed by the ATLAS and CMS collaborations, most of these resulting in smaller uncertainties than those achieved previously. At the same time, huge progress was made on the theoretical side yielding significantly improved predictions up to next-to-next-to-leading order in perturbative QCD. Due to the vast amount of events containing top quarks, a variety of new measurements became feasible and opened a new window to precisions tests of the Standard Model and to contributions of new physics. In this review, originally written for a recent book on the results of LHC Run 1 thisbook (), top-quark measurements obtained so far from the LHC Run 1 are summarised and put in context with the current understanding of the Standard Model.

Originally published in “The Large Hadron Collider — Harvest of Run 1”, edited by T. Schörner-Sadenius, Springer, 2015, pp. 259–300 thisbook ().

## 1 Introduction

Top quarks have been a subject of scientific research ever since Kobayashi’s and Maskawa’s speculations about a third family of quarks in the context of solving the problem of weak violation in the early 1970s Kobayashi:1973fv (). After a two-decade long period of searches at various colliders and experiments, the top quark was finally discovered in 1995 by the CDF and DØ experiments at Fermilab’s Tevatron, a proton-antiproton collider, operated at the time at a centre-of-mass energy of  Abe:1995hr (); Abachi:1995iq (). Since then, and in particular after the upgrade of the Tevatron to a centre-of-mass energy of , pioneering precision measurements were performed at this machine. Prime examples are the measurements of the total cross section for single-top and top-quark pair () production and the measurements of the top-quark mass (see Refs. Aaltonen:2013wca (); Tevatron:2014cka () and references therein). Currently, both CDF and DØ are in the process of publishing their legacy measurements based on data sets corresponding to an integrated luminosity of about collected by each experiment during Tevatron Run 2—and these measurements set a standard for the LHC.

A new era in experimental top-quark physics was marked by the start of the LHC in 2009. At the LHC, top quarks are produced abundantly due to the high centre-of-mass energy, the resulting large rise of the parton luminosities, and the large instantaneous luminosity of the accelerator. During LHC’s Run 1 more than 5 million top-quark events were produced at the collision points in ATLAS and CMS each. Based on these huge data samples, most of the measurements performed at the Tevatron have already been improved and/or complementary studies have been performed. This has only been made possible by inheriting a wealth of analysis techniques from the Tevatron experiments where they were pioneered and brought to perfection. At the LHC, top quarks have become tools for searches for new physics, e.g. the search for rare decays, for measurements of top-quark couplings to gauge bosons, or for the investigation of the proton structure.

In this chapter the experimental findings obtained during LHC Run 1 are summarised and put in context with our current understanding of the Standard Model (SM). Emphasis is placed on three aspects: i) the description of the precision measurements in comparison with results from the Tevatron and with theory predictions, e.g. production cross sections or top-quark properties; ii) the presentation of new measurements that were not performed at the Tevatron and that either improve the current understanding of already measured quantities or enable measurements of yet unexplored processes and quantities, e.g. small couplings or associated production processes; iii) the discussion of the physics lessons and insights gained from the LHC Run 1 results. These results do not only impact on our understanding of the Standard Model, but also help us prepare for future investigations at the LHC and beyond. Several important measurements based on the data from LHC Run 1 are still being performed. This chapter can thus not be complete, and only a selection of the results is presented.

## 2 Top-Quark Pair Production

In hadronic collisions, top-quark pairs are dominantly produced through the strong interaction. At the parton level, the production mechanisms are quark-antiquark annihilation and gluon fusion. Figure 1 shows the corresponding leading-order (LO) Feynman diagrams. The differential cross section for quark-antiquark annihilation can easily be obtained from by replacing the QED coupling with the QCD coupling and introducing an appropriate colour factor (2/9) (see also Chap. 5 of Ref. thisbook ()):

 d^σq¯q→t¯tdz=πα2s9sβ(2−(1−z2)β).

Here denotes the center-of-mass energy squared, is the velocity of the top quark in the partonic centre-of-mass system, is the top-quark mass, and is the cosine of the scattering angle defined as the angle between the incoming quark and the outgoing top quark. The corresponding result for gluon fusion reads

 d^σgg→t¯tdz=πα2s96sβ7+9z2β2(1−z2β2)2(1+2β2−2z2β2−2β4+2z2β4−z4β4).

The hadronic cross section is obtained from the partonic cross section through a convolution with the parton distribution functions (PDFs) which, roughly speaking, describe the probability to find a parton inside a hadron with a momentum fraction between and of the mother hadron. The factorisation scale denotes the scale at which, in higher-order calculations, the initial-state singularities are factorised into the parton distribution functions. The final formula for the hadronic cross section is thus given by

 dσH1H2→t¯t+X = ∑i,j∫dx1dx2fi/H1(x1,μF)fj/H2(x2,μF) (1) × d^σij→t¯t+X(x1P1,x2P2,kt,k¯t,αs(μR),μF),

where , are the momenta of the incoming hadrons, while , are the momenta of the outgoing top quarks. The sum is over all possible partons. The coupling constant is evaluated at the renormalisation scale . Note that in higher order, the partonic cross section also depends on the factorisation scale such that the factorisation scale dependence of the parton distribution functions is cancelled order by order and the hadronic cross section becomes independent of the non-physical scale at fixed order in perturbation theory. For more details we refer to Chap. 5 of Ref. thisbook (). Because the QCD coupling constant is not small (), higher-order corrections can give sizeable contributions and need to be taken into account in most cases. Since the top-quark mass sets a large energy scale, non-perturbative effects are essentially cut off and QCD perturbation theory is believed to give reliable predictions. The next-to-leading order (NLO) QCD corrections for production were calculated a long time ago Nason:1987xz (); Beenakker:1988bq (). Further improvements were obtained by resumming soft-gluon corrections, which lead to a logarithmic enhancement of the cross section, to next-to-leading logarithmic accuracy Catani:1996dj (); Bonciani:1998vc (); Kidonakis:2001nj (). Soft-gluon resummation has been extended recently to the next-to-next-to-leading logarithmic (NNLL) accuracy Kidonakis:2003qe (); Moch:2008qy (); Czakon:2008cx (); Cacciari:2011hy (); Beneke:2011mq (). Despite the fact that top quarks do not form bound states (because of their short lifetime), binding effects still lead to minor corrections of the cross section close to the -pair production threshold. In principle, such a would-be bound state could be observed as a narrow peak in the invariant-mass spectrum, just below the production threshold. However, the energy resolution of the LHC experiments is not sufficient to resolve this effect.111At a future collider, operating at the top-quark production threshold, the effect would be visible thanks to the high energy resolution and could be used for very precise measurements of the top-quark mass. The corresponding corrections to the inclusive cross section are small and have been studied in detail Beneke:2011mq (); Hagiwara:2008df (); Kiyo:2008bv (). Electroweak corrections have also been investigated Beenakker:1993yr (); Kuhn:2005it (); Bernreuther:2005is (); Kuhn:2006vh (); Bernreuther:2006vg (); Hollik:2007sw (); Bernreuther:2008md (). For the inclusive cross section of production at the LHC operating at , they are negative and at the percent level. On the other hand, weak Sudakov logarithms can result in suppression of the cross section at the level of 10–20% for differential distributions at large momentum transfer (see also Chap. 4 of Ref. thisbook ()). Since this region is precisely the one where new heavy resonances could lead to an increase of the cross section, neglecting weak corrections could potentially hide signs of new physics.

Very recently, full next-to-next-to-leading order (NNLO) QCD corrections have been presented for the inclusive cross section Czakon:2013goa (). For a centre-of-mass energy of , the result—including soft-gluon resummation at NNLL accuracy (assuming and the MSTW2008nnlo68cl PDF set Martin:2009iq ())—reads

 σt¯t(√s=8TeV)=245.8+6.2−8.4 (scale)+6.2−6.4 (PDF% ) pb. (2)

Note that the result does not include the aforementioned weak corrections. The first uncertainty is due to the residual222We call the remaining scale dependence “residual” because it is formally of higher order. scale dependence which is used as an estimate of the unknown higher-order contributions. It has been determined by a variation of the renormalisation and factorisation scales in the range . The second uncertainty is due to the incomplete knowledge of the parton distribution functions. From equation (2) we conclude that the total cross section is known with a precision better than 5%. Moving to higher collider energies will slightly improve the PDF uncertainties since less weight is put to the large region where the PDFs are less precisely known.

So far, only very few NNLO results exist for differential distributions. Most predictions are currently restricted to NLO accuracy (extended in some cases by the resummation of soft-gluon corrections). Fixed-order NLO corrections are available, for example, through the parton-level Monte Carlo (MC) program Mcfm Campbell:2012uf (). Combining parton-level NLO calculations with parton-shower simulations is in general not straight forward. A naive combination would count real emission processes twice, since real emission is simulated through the parton shower, but, on the other hand, is also explicitly taken into account in the real-emission processes contributing at NLO. A consistent matching that avoids double-counting has been developed in the past Frixione:2002ik (); Nason:2004rx (). Differential distributions for top-quark pair production at NLO including parton shower effects are given in  Frixione:2003ei (); Frixione:2007nw ().

In all calculations mentioned before, the production of stable top quarks is assumed, which is then followed by an on-shell decay. This corresponds to the “narrow-width” or “double-pole approximation”. The naive expectation is that corrections to this approximation should be suppressed like or even , where denotes the top-quark decay width (see also Ref. Melnikov:1995fx ()). Obviously, the naive expectation can only be true if the observable under consideration is not directly related to off-shell effects. A counter-example is the invariant-mass distribution of the top-quark decay products. Off-shell effects for production have been investigated in detail in Refs. Denner:2010jp (); Denner:2012yc (); Bevilacqua:2010qb (), where the QCD NLO corrections for the process have been calculated. Indeed, the effects are typically small, unless observables of the type mentioned before are studied.

As can be seen from the vast amount of different theoretical studies, production is well understood in the Standard Model. A variety of different corrections have been considered in the past, and precise theoretical predictions for inclusive as well as differential quantities are available. Top-quark pair production is thus an ideal laboratory to test the consistency of the SM and to search for possible deviations. In the following sections we describe the measurements of inclusive and exclusive cross sections for top-quark pair production.

### 2.1 Inclusive t¯t Cross Section

First measurements of the inclusive cross section were published by the ATLAS and CMS collaborations already in the year 2010 Aad:2010ey (); Khachatryan:2010ez (). These are based on data corresponding to an integrated luminosity of about , a fraction of the data collected in 2010. More precise measurements, based on the full 2010 data sample corresponding to an integrated luminosity of became available shortly after Aad:2012qf (); Aad:2011yb (); Chatrchyan:2011nb (); Chatrchyan:2011ew (); Chatrchyan:2011yy ().

The amount of data collected in the years 2011 () and 2012 () correspond to integrated luminosities of about , respectively—altogether more than a factor 500 more than that of 2010. With this wealth of data, top-quark physics entered a completely new realm of precision and detail. With the 2011 data samples, measurements of the inclusive top-quark pair cross section were performed in all decay channels of the system (except the one with two leptons in the final state), reaching an unprecedented level of statistical and systematic precision Aad:2012vip (); Aad:2012mza (); ATLAS:2012aa (); Chatrchyan:2012ria (); Chatrchyan:2012bra (); Chatrchyan:2013ual (); Chatrchyan:2013kff (); Chatrchyan:2012vs (); Khachatryan:2014loa (); Aad:2014jra (); Aad:2014kva ().

In the limit of large statistics, the most precise measurements of the inclusive cross section can be obtained in the - channel, as the backgrounds and associated uncertainties are minimal. The first published measurement of the top-pair cross section at a centre-of-mass energy of was performed by CMS Chatrchyan:2013faa (). It makes use of the decay channel of top-quark pairs with two opposite-charge leptons, one electron and one muon, in the final state. In this channel, backgrounds from non-top-quark events are minimal. Dominant contributions arise from Drell–Yan processes with two leptons in the final state that both decay into a lepton. These backgrounds are suppressed by requiring at least one of the two jets to be -tagged. Smaller background contributions come from single top-quark production (see section 6) and from top-quark events in other decay channels where one of the jets is misidentified as a lepton. In figure 2 the distributions of the -tag multiplicity and the missing transverse momentum after the final event selection are shown. The final result of this measurement is in good agreement with the NNLO prediction quoted in equation (2).

Most recently, the ATLAS collaboration published a measurement yielding the most precise experimental result Aad:2014kva (). In this analysis the numbers of events with exactly one and with exactly two -tagged jets are counted and used to simultaneously determine and the efficiency to reconstruct and -tag a jet from a top-quark decay, thereby minimising the associated systematic uncertainties. In figure 3 the distributions of the -tag multiplicity and the transverse momentum of the -tagged jets are displayed. The cross sections for centre-of-mass energies and are measured to be and respectively, where the latter uncertainty is due to the beam-energy uncertainty.

### 2.2 Differential t¯t Cross Sections

Additional information about top-quark production and decay can be gained from measurements of differential distributions. These do not only probe QCD predictions and provide input to an improved choice of QCD model and scale parameters, but they also have the potential to constrain the parton distribution functions of gluons at large momentum fractions . Moreover, the differential distributions are potentially sensitive to new physics, e.g. to decays of massive -like bosons into top-quark pairs that would become visible at high invariant masses (see also Chap. 11 of Ref. thisbook ()).

The kinematic properties of a top-quark pair are determined from the four-momenta of all final-state objects by means of reconstruction algorithms. For a general introduction to the different decay channels, see e.g. Ref. PT:Top () and references therein. In the single-lepton channels, kinematic-fitting algorithms are applied to obtain the kinematics of both top quarks. In the dilepton channels, due to the presence of two neutrinos, the kinematic reconstruction is under-constrained. Ambiguities between several solutions are resolved by prioritisation, e.g. by the use of the expected neutrino energy distribution.

A large number of distributions of the top quark and the top-quark pair system, as well as their decay products, has been measured at the LHC Aad:2012hg (); Chatrchyan:2012saa (); Aad:2014zka (). In contrast to the situation at the Tevatron, the large production rate at the LHC leads to a substantial reduction of the statistical uncertainties in each bin. The ATLAS and CMS collaborations report normalised differential cross sections, i.e. shape measurements, in which normalisation uncertainties are removed. In figure 4 the distributions of the invariant mass and of the transverse momentum of the top-quark pair system as measured by ATLAS are displayed Aad:2012hg (). The data are very well described by the various calculations up to an energy scale of about . The results from CMS agree with these findings Chatrchyan:2012saa (). The transverse momentum and rapidity distribution of each of the top quarks were also measured and the results from CMS are presented in figure 5. Different theoretical predictions are confronted with the data, and they are generally found to give a good description of the data. However, most Monte Carlo simulations predict the transverse momentum distribution of the top quarks to be somewhat harder than what is seen in the data. This discrepancy between data and simulation is presently under investigation. For the time being it constitutes an important source of uncertainty for many analyses.

### 2.3 Top-Quark Pairs and Additional Jets

At LHC energies, a large fraction of top-quark pairs is accompanied by additional high- jets. Demanding, for example, a minimal transverse momentum of for such additional jets, about 30% of all top-quark pairs are produced together with at least one further jet Dittmaier:2008uj (). From an experimental point of view, the jet activity needs to be understood since the appearance of additional jets affects the event reconstruction. Owing to the large rate, production with jets may also lead to sizeable backgrounds for other SM studies or searches for new physics. As an example, production is the dominant background for Higgs production via vector-boson fusion. From a theoretical perspective, the additional jet activity can be used for further tests of the underlying production and decay mechanisms. Anomalous couplings can be constrained, for example, through a detailed analysis of the process . Assuming the validity of our theoretical understanding, production in association with a jet can also be used to measure the top-quark mass Alioli:2013mxa (). Since the process is proportional to , NLO contributions can easily give corrections of the order of 30%. For a precise understanding it is thus mandatory to take these corrections into account. In Born approximation, the partonic processes , , and contribute to production in association with a jet. The last three processes are related by crossing. The leading-order partonic matrix elements can be calculated e.g. with the help of MadGraph Alwall:2011uj (). The hadronic cross sections are then calculable through a numerical Monte Carlo integration, using again equation (1). For the evaluation of the NLO corrections, the one-loop corrections to the aforementioned Born processes, together with real-emission processes, need to be evaluated. Since the two contributions are individually infrared (IR) divergent—the divergences cancel only in the sum—a method to organise this cancellation needs to be applied. In Refs. Dittmaier:2008uj (); Dittmaier:2007wz (), the one-loop amplitudes have been calculated using a traditional tensor reduction for the one-loop integrals. The cancellation of the IR divergences is achieved using the Catani–Seymour subtraction method Catani:1996vz (); Catani:2002hc (). In Ref. Melnikov:2010iu (), an alternative calculation of the NLO corrections, based on the unitarity method, has been presented. In a subsequent study Melnikov:2011qx (), also the on-shell decay of the top quark has been taken into account. NLO results for production in association with a photon are also available at NLO QCD Melnikov:2011ta (), since this process is closely related to production in association with jets. In figure 6(a), the cross section for production is shown as a function of the renormalisation scale which is set equal to the factorisation scale. For the parton distribution functions the CTEQ6 set Pumplin:2002vw () has been used.

The transverse momentum of the additional jet is required to be at least . The leading-order result strongly depends on the renormalisation scale , a fact that directly reflects the running of the coupling constant . The Born approximation can thus at best be considered as a rough estimate of the cross section. The NLO corrections as a function of the renormalisation scale, however, show a flat behaviour around . This may be considered as an indication that provides a natural scale for this process. It can also be seen from figure 6(a) that the corrections are rather small for . Similar observations can be made in figure 6(b) where the rapidity distribution of the additional jet, calculated at NLO, is shown. In Refs. Dittmaier:2008uj (); Melnikov:2011ta () a large variety of differential distributions have been investigated. In particular the transverse momentum distribution of the top quark, the system and the additional jet have been calculated. It turns out that for large transverse momentum , significant QCD corrections together with a large scale uncertainty are observed. In principle, this is not surprising since at a large transverse momentum an additional scale—different from —is introduced. It is conceivable that a phase-space-dependent renormalisation scale could improve the behaviour of the perturbation theory by effectively resumming large logarithmic corrections. In table 1, the dependence of the cross section on the required minimal transverse momentum of the additional jet, , is shown. A strong dependence on is found. For the cross section diverges logarithmically (the divergence cancels a similar divergence in the cross section for inclusive production at NNLO, when production is combined with the two-loop corrections to inclusive production).

With the exception of , where very small and negative corrections are observed, the corrections are positive and typically about 15–20%.

Recently, NLO corrections for production in association with two additional jets were studied. For details, we refer to the original work Bredenstein:2009aj (); Bredenstein:2008zb (); Bredenstein:2010rs (); Bevilacqua:2011aa (); Bevilacqua:2012em (); Hoeche:2014qda ().

The ATLAS and CMS collaborations studied the distributions of jet multiplicities and additional jets due to QCD radiation in detail Chatrchyan:2014gma (); ATLAS:2012al (); Aad:2014iaa (). The multiplicity distributions of jets for events in the single-lepton channel as measured by the CMS collaboration is shown in figure 7. The data are generally well described by the Monte Carlo predictions obtained using MadGraph, Powheg and MC@NLO. Towards very large multiplicities, the MC@NLO generator interfaced with parton showers from Herwig predicts significantly less events than MadGraph or Powheg, which both use Pythia to generate the parton showers.

An alternative way of investigating additional activity in events is to study “gap-fraction” distributions Chatrchyan:2014gma (); ATLAS:2012al (). In these studies, events are vetoed if they contain an additional jet with transverse momentum above a given threshold in a central rapidity interval. The fraction of events surviving the jet veto, the gap fraction, is presented as a function of the threshold. The gap-fraction distributions for jets as measured by ATLAS are displayed in figure 8. A qualitatively similar trend is observed as in the multiplicity distribution (figure 7) in that the MC@NLO generator predicts a larger fraction of events that have no jet activity beyond the jets originating directly from the top-quark decays. However, vetoing jets just in the forward region, at rapidities , all simulations predict a smaller fraction of events with no additional jet than is seen in the data. These results can be used to improve the choice of models, scale parameters and tunes in Monte Carlo simulations for an optimal description of the data.

Building up on the insights about inclusive distributions of additional jets in top-quark pair events, both ATLAS and CMS have also been studying distributions and rates of events with additional jets originating from heavy quarks. These form an important background to events in which Higgs bosons are produced in association with top-quark pairs, with subsequent decay of the Higgs boson into or pairs, see Chap. 6 of Ref. thisbook (). The ATLAS experiment published a measurement of top-quark pairs together with heavy-flavour quarks, or at  Aad:2013tua (). The separation between heavy-flavour and light-flavour contents of additional jets is achieved by a fit to the vertex-mass distribution of -tagged jets, shown in figure 9. From the fit, the relative contribution of heavy quarks is extracted to be , consistent within uncertainties with leading-order expectations, see Ref. Aad:2013tua () and references therein.

## 3 Top-Quark Mass

In the SM, the couplings of the top quark to the gauge bosons are governed by the gauge structure (see also Chap. 4 of Ref. thisbook ()). The only free parameters in top-quark physics are thus the three corresponding CKM matrix elements and the top-quark mass, . Instead of the top-quark mass, one may also use the Yukawa coupling to the Higgs boson as a free parameter since the two are related by , where is the vacuum expectation value of the Higgs field. Once the CKM matrix elements and the top-quark mass are known, the SM makes testable predictions for all top-quark properties. Precise measurements of these properties can thus be used to test the consistency of the SM. A prominent example is provided by the simultaneous measurements of the top-quark mass, the -boson mass and the mass of the Higgs boson since these three masses are related in the SM: The -boson mass can be calculated as a function of the top-quark mass and the mass of the Higgs boson. A comparison with the measured values thus allows the mechanism of electroweak symmetry breaking predicted by the SM to be indirectly tested. This is demonstrated in figure 10 where, for comparison, also results within the minimal supersymmetric Standard Model (MSSM, see e.g. Chap. 10 of Ref. thisbook ()) are shown Heinemeyer:2013dia ().

Recently, also the question of vacuum stability has attracted a lot of attention (see for example Refs. Degrassi:2012ry (); Degrassi:2014hoa ()). Through quantum corrections, the top quark influences the effective Higgs potential that is responsible for electroweak symmetry breaking. In principle, it is conceivable that these quantum corrections modify the effective potential such that it develops a second minimum or even becomes unbounded from below. As a consequence, the electroweak vacuum might become metastable or even unstable. Calculating the corresponding lifetime of the vacuum and comparing it with the age of the universe provides a further consistency test of the SM.

Experimentally, in most measurements, the mass of the top quark is determined through the reconstruction of the top quark’s decay products. The top-quark mass can be estimated by comparing the measured values with the value of the mass parameter used in the simulation. Measurements employing this approach generally achieve the most precise results.

In contrast, from a theoretical point of view, a meaningful definition of the top-quark mass requires to specify the renormalisation scheme used to define the parameter in the theoretical predictions. In this respect the top-quark mass should be treated similar to a coupling constant. In the theoretical description of hadronic collisions, the so-called “on-shell” or “pole mass” scheme and the “minimal subtraction scheme” () are commonly used. Quantitatively, the pole mass and the mass measured from final state reconstruction are expected to agree within  Buckley:2011ms (); Moch:2014tta ().

In the pole mass scheme, the renormalised mass is defined as the location of the pole of the renormalised quark propagator, including higher-order corrections. In the (modified) minimal subtraction scheme, the renormalised parameters are defined through a minimal subtraction of the ultraviolet (UV) divergences. The renormalisation constants are chosen such that they just cancel the UV divergences encountered in the loop corrections (together with some irrelevant transcendental constants in the modified minimal subtraction scheme). The two definitions are related in perturbation theory. At NLO accuracy, for example, the relation reads

 mpolet=¯mt(μR){1+αs(μR)πCF[1−34ln(¯mt(μR)2μ2R)]}, (3)

where defines the pole mass and defines the mass in the modified minimal subtraction scheme. denotes the Casimir operator in the fundamental representation. The mass depends on the renormalisation scale, which coins the term “running mass”.

The pole mass scheme is closely related to the intuitive understanding of the mass of a free particle. While for many applications this intuitive picture is a good approximation—for many purposes the top quark behaves like a free quark—it should be clear that this picture is doomed to fail if it comes to ultimate precision. Indeed, it has been shown that the pole mass suffers from the so-called “renormalon ambiguity” that leads to an intrinsic uncertainty of the pole mass of the order of  Bigi:1994em (); Beneke:1994sw (). Despite the fact that the pole mass and the mass definitions are related in perturbation theory, it is in practice not straightforward to convert theoretical results from one scheme to the other. So far, this translation has only been calculated for the inclusive cross section for production and for a few differential distributions in production.

Experimentally, the top-quark mass has been measured at the LHC using a large variety of methods and observables, and in different decay channels ATLAS:2012aj (); Chatrchyan:2012ea (); Chatrchyan:2013boa (); Chatrchyan:2013xza (); Chatrchyan:2012cz (); Chatrchyan:2011nb (); Aad:2014zea (). In addition, the difference of the masses of top quarks and antiquarks have been measured Chatrchyan:2012uba (); Aad:2013eva ().

A recent measurement using events with fully hadronic final states is presented by the ATLAS collaboration Aad:2014zea (). Events are selected if they contain at least six jets, and exactly two -tagged jets are required to be among the four leading jets. The top-quark mass is extracted from a binned likelihood fit to the distribution, shown in figure 11, where is the ratio of the reconstructed three-jet and two-jet masses. In this distribution systematic effects that are common to the masses of the reconstructed top quark and the associated boson cancel. The contribution from multi-jet backgrounds is determined from the data using the event yields in different regions of -tag jet multiplicity and 6th-jet momentum. The measurement yields a value for the top-quark mass of

 mt=175.1±1.4 (stat)±1.2 (syst)GeV.

The systematic uncertainties are dominated by the residual uncertainties of the jet energy scale, in particular for -quark jets, and by the uncertainties from hadronisation modelling.

The CMS collaboration presented a measurement of the top-quark mass using the full data set collected at a centre-of-mass energy of with one electron or muon and at least four jets in the final state Chatrchyan:2012cz (). A kinematic fit to the four leading jets, the lepton and the missing transverse momentum is employed to constrain the selected events to the hypothesis of the production of two heavy particles of equal mass, each one decaying to a boson and a quark. The reconstructed masses of the two bosons are constrained in the fit to . The reconstructed invariant-mass distribution is shown in figure 12. Events can enter the distributions with different parton-jet assignments (permutations). For simulated events, the parton-jet assignments can be classified as correct, wrong and unmatched permutations where, in the latter, at least one quark from the decay is not matched to any of the four selected jets. The actual top-quark mass value is determined simultaneously with the jet energy scale using a joint likelihood fit. The joint likelihood is constructed based on the “ideogram method” in which the likelihood for each event is evaluated from analytic expressions obtained from simulated events. Biases arising due to this method are determined using pseudo-experiments and corrections are applied accordingly. The dominant uncertainty of the final result comes from the uncertainty of the difference in the jet energy responses for jets originating from light (, , ) or bottom quarks, as well as from statistical uncertainties in the determination of differences between different models for colour-reconnection processes. The final result is

 mt=173.49±0.43 (stat+JES)±0.98 (syst)GeV,

corresponding to an optimal jet energy scale correction of with respect to the CMS calibration.

In spring 2014, this and other precise results from the LHC and the Tevatron, both preliminary and final, were combined to obtain a first world average of the top-quark mass ATLAS:2014wva (). A summary is shown in figure 13.

An alternative approach to the determination of the top-quark mass is to extract its value from the measured inclusive cross section. This approach has the advantage that the cross section and the pole mass are directly related, such that the extraction yields a theoretically well-defined quantity. Both ATLAS and CMS have used their cross-section measurements to extract the top-quark pole mass Chatrchyan:2013haa (); Aad:2014kva () as defined at NNLO accuracy Czakon:2013goa (). The extractions are performed for different parton distribution functions and take into account the experimental dependence of the measured cross section on the assumed top-quark mass. A summary of the results is shown in figure 14.

Conversely, assuming equality between the pole mass and the directly measured mass within , the cross-section measurements can be used to determine the strong coupling constant  Chatrchyan:2013haa ().

## 4 Tests of QCD Predictions

Perturbative QCD (pQCD) is a fundamental building block for the understanding of physics processes at the LHC. In addition to cross-section predictions, several other aspects of pQCD can be probed in the top-quark sector. Examples are the small but finite charge asymmetry of pairs and the correlation between the top-quark and antiquark spins in production; both quantities are sensitive to the relative proportions of the different production processes of pairs. Another example is the polarisation of top quarks in events, which tests the and structure of production.

### 4.1 Charge Asymmetry

At leading order QCD, the reactions and are symmetric under the exchange of top quarks and antiquarks. The relevant hard scattering processes are quark-antiquark annihilation, , and gluon-fusion, . At NLO, two additional types of processes have to be considered which break this charge symmetry, namely quark-gluon scattering, , and radiative corrections to quark-antiquark annihilation Kuhn:1998jr (); Kuhn:1998kw (). In both cases, the charge asymmetry is induced by interference effects, e.g. interference between processes with initial-state and final-state radiation or interference between Born and box diagrams. All gluon-fusion processes are symmetric under the exchange of the top quark and antiquark.

The charge asymmetry results in an asymmetry of the event kinematics: Top quarks (antiquarks) are preferentially emitted in the direction of the incoming quark (antiquark). The observables with which the charge asymmetry can be measured are chosen depending on the colliding particles and the centre-of-mass energy. Quark-antiquark annihilation dominates the production of pairs at the Tevatron, and so the top quark and antiquark will preferentially be emitted in the direction of the incoming protons and antiprotons, respectively. The most common observable is thus a forward-backward asymmetry,

 At¯t=N(Δy>0)−N(Δy<0)N(Δy>0)+N(Δy<0),

where is the difference between the rapidities of the top quark and antiquark, i.e. , and is the number of events. The predictions for this observable depend on several kinematic variables. The inclusive forward-backward asymmetry is predicted to be  Bernreuther:2012sx (), while for invariant masses larger than the prediction increases to  Bernreuther:2012sx (). The CDF and DØ experiments have measured the forward-backward asymmetry both inclusively and as a function of several kinematic quantities, e.g.  Aaltonen:2012it (); Abazov:2011rq (). They found an excess compared to the NLO QCD predictions with significances of several standard deviations. Over the last few years these measurements gave rise to speculations about contributions to production due to physics beyond the Standard Model. Although refined theoretical studies and further measurements appear to have resolved the issue, measurements of the charge asymmetry are still in the focus of the LHC top-physics programme.

At the LHC with its symmetric initial state, the charge asymmetry can not be measured as a forward-backward asymmetry. Instead, a central-decentral asymmetry is defined. As valence quarks carry a larger average momentum fraction and top (anti)quarks are produced preferentially in the direction of the incoming (anti)quark, the average top-quark rapidity is larger than that of top antiquarks. A useful observable is defined as

 AC=N(Δ|y|>0)−N(Δ|y|<0)N(Δ|y|>0)+N(Δ|y|<0),

where is the difference between the absolute values of the top-quark and top-antiquark rapidities, i.e. . The NLO QCD prediction including electroweak effects for the inclusive asymmetry is  Bernreuther:2012sx (). Predictions are also available for different values of the invariant mass, the rapidity and the transverse momentum of the pair, and they range between -0.6% and 2.8% (see discussion in Ref. Aad:2013cea ()). The asymmetry depends on the first two variables because they are correlated to the fraction of quark-antiquark annihilation in production. It depends on the latter quantity because the amount of initial-state and finale-state radiation changes with increasing transverse momentum.

After an initial measurement using only a subset of the available data recorded at  ATLAS:2012an (), the ATLAS collaboration has studied the charge asymmetry based on the full data set, which corresponds to an integrated luminosity of  Aad:2013cea (). Events are selected that are consistent with the single-lepton decay mode of production. For each event, the top-quark pair is reconstructed using a likelihood-based kinematic fit Erdmann:2013rxa (), and the rapidities of the top quark and antiquark are reconstructed. The measured distribution of includes background events and is distorted by detector and acceptance effects. A Bayesian unfolding technique Choudalakis:2012hz () is applied on the background-subtracted spectrum to remove such effects. The measured inclusive asymmetry is

 AC=0.006±0.010,

where the largest sources of uncertainty are the statistical uncertainty and the uncertainty due to lepton and jet reconstruction. In addition, the asymmetry for invariant masses greater than is found to be which is in good agreement with the predicted value of . The asymmetry is also measured as a function of the transverse momentum, the absolute value of the rapidity and the invariant mass of the pair. The latter measurement is repeated for a subset of the events featuring a high longitudinal velocity, i.e. requiring . The asymmetries as a function of the invariant mass are shown in figure 15 without (a) and with (b) the additional velocity requirement. All four differential measurements are in agreement with the SM predictions.

The CMS collaboration has measured the charge asymmetry in a data set corresponding to an integrated luminosity of  Chatrchyan:2011hk (); Chatrchyan:2012cxa () using events with exactly one charged lepton in the final state. After event reconstruction and calculation of the top-quark and top-antiquark rapidities, the distribution is determined. Subsequently, the estimated background contributions are subtracted from the data and the spectra are corrected for detector and acceptance effects using a regularised unfolding procedure via matrix inversion Blobel:2002pu (). The measured inclusive asymmetry is

 AC=0.004±0.010 (stat)±0.011 (% syst),

where the major sources of systematic uncertainty are the residual model dependence of the unfolding procedure and the lepton reconstruction. As in the ATLAS measurement, the asymmetry is also measured as a function of the transverse momentum, the rapidity and the invariant mass of the system. Figure 16(a) shows the background-subtracted and unfolded distribution for the inclusive case, and figure 16(b) shows the charge asymmetry as a function of the transverse momentum of the pair. All measurements are consistent with the SM predictions.

In a further study using the full data set, the CMS collaboration measured the charge asymmetry in a sample of dileptonically decaying pairs Chatrchyan:2014yta (). In addition to the observable , a “lepton charge asymmetry” is defined as

 AlepC=N(Δ|ηℓ|>0)−N(Δ|ηℓ|<0)N(Δ|ηℓ|>0)+N(Δ|ηℓ|<0),

where and where are the pseudo-rapidities of the positively and negatively charged leptons in each event. The SM prediction for this observable is  Bernreuther:2012sx (). The event reconstruction is performed using the “analytical matrix weighting technique” (AMWT) Chatrchyan:2011nb (). After subtracting all background contributions from the measured and distributions, the spectra are unfolded using singular value decomposition Hocker:1995kb (). The measured asymmetries are

 AC = −0.010±0.017 (stat)±0.008 (syst) and AlepC = −0.009±0.010 (stat)±0.006 (syst),

where the largest sources of systematic uncertainty are residual biases in the unfolding procedure and uncertainties in the modelling and the jet reconstruction. The lepton charge asymmetry is also calculated as a function of the same three kinematic variables as for the single-lepton analysis. No deviations between the measurements and the predictions are found.

The charge asymmetry in production is predicted to cause a small effect on a variety of observables at the LHC. None of the measurements performed by the ATLAS and CMS collaborations are in conflict with the SM predictions while the current experimental precision is of the order of the size of the prediction itself. Although a variety of models of physics beyond the Standard Model can be excluded with the set of measurements already performed, the analysis of the data (which was not finished at the time of publication) will provide further sensitivity to the predictions of perturbative QCD. It should be noted, that the interpretation of the leptonic charge asymmetries relies on a solid understanding of top-quark production and decay. In particular, a non-standard top-quark polarisation could affect the leptonic asymmetries. It is thus important to cross check the polarisation through explicit measurements.

### 4.2 Top-Quark Polarisation and Spin Correlation in Top-Quark Pairs

Top-quark polarisation in events and the correlation between the top-quark and antiquark spins in production are probes of perturbative QCD and observables that are sensitive to anomalous production mechanisms. Measurements of such quantities are only feasible because of the extremely short lifetime of the top quark of . The lifetime is roughly one order of magnitude smaller than the time scale at which hadronisation takes place, , and in particular shorter than the time needed to decorrelate the spin configuration of the pair,  Grossman:2008qh (); Mahlon:2010gw (). Top quarks will thus decay before they can form bound states. As mentioned before, the large top-quark width cuts off non-perturbative effects. The polarisation of the top-quark is thus not diluted by hadronisation effects and can be calculated reliably within perturbation theory. The parity-violating weak decay can then be used to analyse the top-quark polarisation through the angular distribution of the decay products. The correlation of the top-quark and antiquark spins is reflected in the angular correlation of the top-quark and antiquark decay products. This is a unique feature since all lighter quarks form hadrons for which—due to the hadronisation process—the initial spin information of the mother particle is diluted or even entirely lost. In contrast, the spin information of the top quark is directly transferred to its decay products.

In top-quark pairs, information about the polarisation of top quarks and the correlation between top-quark and antiquark spins can be obtained from the differential cross section

 1σdσdcos(θ1)dcos(θ2) = 14(1+α1P1cos(θ1)+α2P2cos(θ2) (4) −α1α2Acos(θ1)cos(θ2)),

where () are the angles between the momentum direction of a daughter particle of the top (anti)quark and a chosen reference axis. The coefficients () and () are the “spin-analysing power” of the daughter particle and the degree of polarisation (with respect to the reference axis) of the top (anti)quark, respectively. The spin-analysing power quantifies the amount of spin information transferred to the daughter particle and depends on the particle type. It is approximately one for charged leptons and down-type quarks from the subsequent decay of the boson Brandenburg:2002xr (). The coefficient is a measure of the spin correlation between top quark and antiquark.

As the strong interaction conserves parity, the polarisation of top (anti)quarks in production within the production plane is expected to be zero. QCD absorptive parts, sometimes also called final-state interactions333These are due to imaginary parts of the loop integrals caused by the on-shell production of intermediate states., introduce a tiny transverse polarisation at the one-loop level Bernreuther:1995cx (); Dharmaratna:1989jr (). Electroweak corrections lead to a small amount of net polarisation of  Bernreuther:2013aga (). It can be shown that polarisation can be induced by the imaginary part of a chromo-electric dipole moment which in turn can lead to -odd and -odd terms in the matrix elements Bernreuther:2013aga (). Such effects can stem from processes beyond the SM.

The correlation coefficient can be expressed as an asymmetry variable in the number of events with parallel and antiparallel spin,

 A=N(↑↑)+N(↓↓)−N(↑↓)−N(↓↑)N(↑↑)+N(↓↓)+N(↑↓)+N(↓↑),

where and indicate the spin projections onto the reference axis. The prediction of the correlation coefficient depends on the particular choice of reference axis. While for measurements at the Tevatron the “off-diagonal basis” and the “beam basis” are suitable choices, measurements at the LHC are most sensitive to the correlation coefficient in the “helicity basis”. In the beam basis, the direction of the beam is used as reference axis for the top-quark as well as for the antiquark. In the helicity basis, the direction of flight of the top-quark/antiquark is used as respective reference axis. The strength of the correlation predicted by the SM using the helicity basis is  Bernreuther:2010ny () with an uncertainty of approximately 1%.

Close to the threshold, top-quark pairs produced via gluon fusion are in a state while top-quark pairs produced via quark-antiquark annihilation are in a state. As a consequence, the spins of a top-quark pair produced in quark-antiquark annihilation tend to be parallel while in gluon fusion they tend to be antiparallel. A measurement of the coefficient is thus a direct probe of the production mechanism. Contributions from additional production mechanisms, e.g. yet unknown intermediate vector bosons, can lead to altered predictions for . Note that the correlation coefficient depends both on the centre-of-mass energy and on the initial-state particles, and so the measurements conducted at the Tevatron and the LHC are complementary.

While an evidence for correlated spins in top-quark pairs was already reported by the DØ collaboration Abazov:2011gi (), the hypothesis that the spins of the top quark and the antiquark are uncorrelated was fully disproved for the first time by a measurement of the ATLAS collaboration ATLAS:2012ao (). The measurement is based on a data set corresponding to an integrated luminosity of recorded at . Events consistent with the signature of events decaying in the dilepton mode are selected, and the spin correlation is probed using the difference in azimuthal angle between the two charged leptons, , calculated in the laboratory frame. The advantage of this observable compared to those in equation (4) is that no kinematic reconstruction of the top-quark momenta is necessary while the sensitivity to the correlation strength is largely retained Mahlon:2010gw (). Figure 17(a) shows the observed spectrum as well as the predictions for the assumption of SM correlations and the absence of correlations. The measured correlation coefficient is not compatible with zero,

 A=0.40±0.04 (stat)+0.08−0.07 (syst),

with a significance of 5.1 standard deviations. The dominating sources of systematic uncertainty are the estimate of events with misidentified leptons and the jet reconstruction. In a second publication based on the full data set Aad:2014pwa (), the spin correlation is measured in the dilepton channel using a variety of alternative observables, and it it also measured in the single-lepton channel.

The CMS collaboration has analysed a data set corresponding to an integrated luminosity of recorded at  Chatrchyan:2013wua (). Events are selected that contain exactly two charged leptons with large transverse momenta. Three angular variables are calculated for each event—the variable defined earlier as well as the angles and , which are defined as the angles of the positively and negatively charged lepton in the helicity frame, respectively. From the distributions of these variables, two asymmetries are derived which provide discrimination between the two scenarios of SM correlations and no correlations:

 AΔϕ = N(Δϕ>π/2)−N(Δϕ<π/2)N(Δϕ>π/2)+N(Δϕ<π/2), Acoscos = N(cos(θℓ+)cos(θℓ−)>0)−N(cos(θℓ+)cos(θℓ−)<0)N(cos(θℓ+)cos(θℓ−)>0)+N(cos(θℓ+)cos(θℓ−)<0).

The latter asymmetry is a measure for the correlation coefficient in the helicity basis, i.e.  Bernreuther:2013aga (). The predictions at NLO perturbation theory for the case of SM-like correlations (no correlations) are () and (), see Refs. Bernreuther:2010ny (); Bernreuther:2013aga () and references in Ref. Chatrchyan:2013wua (). The angles require the explicit reconstruction of both the top quark and the antiquark, which is done using the AMWT technique. In addition, the relation between the asymmetry variable and the correlation coefficient is valid only if no acceptance cuts and detector effects distort the measurement. The distributions of and are thus unfolded using singular value decomposition. Figure 17(b) shows the unfolded distribution and the predictions for the two correlation scenarios. The asymmetries are measured to be

 AΔϕ = −0.133±0.010 (stat)±0.007 (syst)±0.012 (top pT) and Acoscos = −0.021±0.023 (stat)±0.027 (syst)±0.010 (top pT),

where the statistical and systematic uncertainties as well as an uncertainty associated with the modelling of the spectrum of the top quark are given. The largest systematic uncertainties come from the unfolding procedure as well as the jet reconstruction, the background estimate and the modelling of events.

The measurements conducted by ATLAS and CMS show that the spins of the top quark and the antiquark in events are indeed correlated and that the amount of correlation is as expected from perturbation theory at NLO. The production mechanisms of events is thus consistent with that predicted by QCD, and no indications for additional production mechanisms are found.

The polarisation of top quarks in events is studied by CMS using the same data set and event selection as for the measurement of the spin correlation Chatrchyan:2013wua (). The polarisation is estimated from the unfolded distribution of the angle and the resulting asymmetry,

 AP=N(cos(θℓ)>0)−N(cos(θℓ)<0)N(cos(θℓ)>0)+N(cos(θℓ)<0).

The polarisation in the helicity basis is then . The asymmetry is calculated using positively and negatively charged leptons under the assumption of invariance and is measured to be

 AP=0.005±0.013 (stat)±0.020 (syst)±0.008 (top pT),

where the uncertainties are again the statistical and systematic ones and the uncertainty due to the mismodelled spectrum of the top quark. The two largest systematic uncertainties are uncertainties on the top-quark mass and on the jet reconstruction.

An ATLAS measurement of the top-quark polarisation Aad:2013ksa () uses events decaying in the single-lepton and dilepton mode. The data were collected at and correspond to an integrated luminosity of . The full system is reconstructed using a kinematic likelihood Erdmann:2013rxa () in the single-lepton channel and the neutrino-weighting method Abbott:1997fv () in the dilepton channel. The angle is calculated in the helicity basis for each lepton, and the corresponding distributions are fitted with templates of partially polarised top quarks. The spin correlation is assumed to be that of the SM. The fits are done separately for each lepton type as well as for positively and negatively charged leptons. The latter is done in order to distinguish scenarios in which the polarisation comes from -conserving processes and maximally -violating processes. For such cases, the expressions are either the same for top quark and antiquark, or they differ by a sign. Figure 18 shows the distributions of measured in single-lepton events for the two scenarios. The combined polarisation measured for the two scenarios is

 αℓP = −0.035±0.014 (stat)±0.037 (syst) % (CP invariance), αℓP = −0.020±0.016 (stat)+0.013−0.017 (syst) (CP violation).

The major systematic uncertainty stems from the jet reconstruction.

The ATLAS and CMS measurements are both consistent with the SM prediction that top quarks produced in pairs via the strong interaction are not polarised.

## 5 Tests of Electroweak Predictions

Studies of the electroweak couplings of the top quark comprise measurements of a number of different observables. While the polarisation of bosons from top-quark decays is a consequence of the structure of the vertex, the cross sections for single top-quark production depend directly on the strength of the coupling to bosons (see section 6). The coupling strength to bosons and photons can be probed by measurements of production with additional such bosons.

### 5.1 W-Boson Polarisation

The massive bosons produced in top-quark decays are real spin-1 particles and thus have three possible polarisation states. We will refer to them as longitudinally, left-handedly or right-handedly polarized bosons. The net amount of polarisation is given by the fractions of the partial decay widths for differently polarised bosons, , and , respectively. These “helicity fractions” are

 F0/L/R=Γ0/L/RΓ0+ΓL+ΓR.

In perturbation theory at LO, and neglecting the mass of the bottom quark, these fractions depend solely on the masses of the top quark and the boson, i.e.

 F0 = m2tm2t+2M2W≈0.70, FL = 2M2Wm2t+2M2W≈0.30, FR = 0.

Calculations at NNLO that include electroweak corrections and assume a finite mass of the bottom quark yield , and  Czarnecki:2010gb (). The helicity fractions can be altered if the structure of the vertex differs from a pure coupling. Such deviations are typically described by anomalous couplings in effective field theory approaches AguilarSaavedra:2006fy (); Zhang:2010dr ().

Information about the polarisation of the boson can be obtained from angular distributions of the final-state particles. In the single-lepton and dilepton channels of production, the angle is defined as the angle between the reverse momentum of the leptonically decaying top quark and the direction of the charged lepton, both evaluated in the rest frame of the corresponding boson Kane:1991bg (). The differential decay width can then be written as

 1ΓdΓdcos(θ∗) = sin(θ∗)2F0+38(1−cos(θ∗))2FL (5) +38(1+cos(θ∗))2FR.

An angle for the hadronically decaying top quark can be defined analogously. The ATLAS and CMS collaborations have both made use of the angular dependence described by equation (5) to estimate the helicity fractions.

The ATLAS collaboration has analysed a data set corresponding to an integrated luminosity of taken at a centre-of-mass energy of  Aad:2012ky (). Two sets of selection criteria are defined so as to enrich samples with events stemming from production with subsequent decay either in the single-lepton or dilepton decay modes. In both cases, the reconstruction of the top quarks is based on the final-state particles and assumptions on the detector performance. For both event types, an individual analysis strategy is followed. While the first strategy is based on a template fit of the distributions, the second makes use of the angular asymmetries derived from unfolded spectra. The individual results are all found to be in agreement and are combined using the BLUE method Valassi:2003mu (). Although both analysis methods are based on the same data set, the combined result has a smaller overall uncertainty due to the different sensitivities to sources of systematic uncertainty. The largest systematic uncertainties are due to the signal and background modelling, to the jet reconstruction and to method-specific uncertainties. The combined helicity fractions are

 F0 = 0.67±0.03 (stat)±0.06 (syst), FL = 0.32±0.02 (stat)±0.03 (syst), FR = 0.01±0.01 (sta.)±0.04 (syst),

with a correlation between and of .

The CMS collaboration has analysed the full data set corresponding to an integrated luminosity of  Chatrchyan:2013jna (). Events are selected that are compatible with the single-lepton decay mode, and top quarks are reconstructed from the final-state particles using a constrained fit. An estimate of the helicity fractions is obtained using a reweighting procedure and a subsequent fit to the distribution. The largest sources of systematic uncertainty are the background estimate and the jet reconstruction. The helicity fractions are estimated to be

 F0 = 0.682±0.030 (stat)±0.033 (syst), FL = 0.310±0.022 (stat)±0.022 (syst), FR = 0.008±0.012 (stat)±0.014 (syst),

with a correlation between and of . A more recent measurement of the helicity fractions using a data sample collected at and enriched with single top-quark events is in good agreement with these values Khachatryan:2014vma ().

The results obtained by the ATLAS and CMS collaborations are consistent with one another and with the NNLO predictions. Both measurements are more precise than those published by Tevatron experiments.

The measured helicity fractions are also interpreted in terms of anomalous couplings. Figure 19(a) shows the 68% and 95% CL contours in the plane of the (real) tensor couplings and assuming vector couplings of and as obtained by the more precise CMS result. A second region of solutions featuring large values of the real part of is excluded from the fit as it is not compatible with the measurement of the single-top -channel cross section. The results are consistent with the absence of anomalous couplings, i.e. , and are in very good agreement with the predicted structure of the vertex.

### 5.2 Top-Quark Pairs and Additional Gauge Bosons

While the production of a top-quark pair and an additional photon has only been observed at the Tevatron Aaltonen:2011sp (), the CMS collaboration was the first to measure the production of top-quark pairs with additional bosons () and bosons (Chatrchyan:2013qca (); Khachatryan:2014ewa (). Such rare processes are expected in the SM. For a centre-of-mass energy of , calculations at NLO yield predictions for the corresponding cross sections  Garzelli:2012bn () and  Campbell:2012dh () of

 σt¯tZ = 0.137+0.012−0.016pb, σt¯tW = 0.169+0.029−0.051pb.

Here the analysis at TeV is briefly described Chatrchyan:2013qca (). The data set collected corresponds to an integrated luminosity of . Events are selected according to the number of charged leptons in the final state. The process

 pp→t¯tZ→(t→bℓ±ν)(t→bjj)(Z→ℓ±ℓ∓)

is searched for by requiring two leptons with the same flavour but opposite electric charge and with an invariant mass compatible with the mass of the boson, and one additional charged lepton. After the event selection, nine events are observed while background events are expected. The resulting cross section is estimated to be

 σt¯tZ=0.28+0.14−0.11 (stat)+0.06−0.03 (syst)pb,

where the dominant source of systematic uncertainty is the background yield.

On the other hand, the processes

 pp → t¯tZ→(t→bℓ±ν)(t→bjj)(Z→ℓ±ℓ∓), and pp → t¯tW→(t→bℓ±ν)(t→bjj)(W→ℓ±ν)

are searched for by selecting events with exactly two leptons of the same electric charge. After the event selection, 16 events remain, while the background expectation is . The combined cross section, , where , is measured as

 σt¯tV=0.43+0.17−0.15 (stat)+0.09−0.07 (syst)pb.

Both measurements and their NLO predictions are shown in figure 19(b). The measured cross sections are in agreement with the predictions, which indicates that no deviation from the strength of the top-quark coupling to and bosons predicted by the SM is observed. The results from the more recent CMS analysis at  Khachatryan:2014ewa () are also consistent with this conclusion.

## 6 Single Top-Quark Production

Single top-quark production, in contrast to top-quark pair-production which proceeds through the strong interactions, takes place by virtue of charged-current interactions. The production rate for single top quarks is suppressed with respect to top-quark pair production by a factor of 2–3 due to the different couplings strengths and of weak and strong interactions, which is only partially compensated by the larger partonic fluxes due to the lower production threshold. Feynman diagrams of the LO processes contributing to the scattering amplitudes are shown in figure 20.

Depending on whether the boson is space-like (figure 20(a)), time-like (figure 20(b)) or real (figure 20(c,d)), one distinguishes between the -channel, the -channel and the -channel. In the latter case, a single top quark is produced in association with a boson in the final state. The dominant contribution to single top-quark production at the Tevatron and the LHC is the -channel. As can be seen from figure 20(a), this channel assumes the existence of a quark inside the proton and thus requires in the theoretical description the so-called five-flavour scheme, in which are treated as active flavours inside the proton. In the four-flavour scheme, -channel production occurs formally at higher orders of the QCD coupling, as is illustrated in figure 21.

In general, calculations in these two schemes should give similar results. Differences occur if logarithmic corrections of the form become large, where denotes a generic energy scale. The five-flavour scheme may partially resum these logarithms through the evolution of the -quark parton distribution function, while in the four-flavour scheme these logarithms are kept at fixed order only. In Refs. Campbell:2009ss (); Campbell:2009gj () it has been checked through an explicit calculation that the two schemes lead indeed to consistent results for the cross section.

At the LHC, the second important production channel for single top quarks is the channel. Due to phase-space suppression and the small gluon luminosity, this channel gives only a tiny contribution at the Tevatron. In contrast, -channel production, which is roughly responsible for one third of the cross section at the Tevatron, leads only to a contribution of a few percent at the LHC. Single top-quark production at the LHC is thus to some extent complementary to that at the Tevatron. A further major difference arises from the fact that the initial state at the Tevatron is a eigenstate. Since -violating effects are negligible in single top-quark production within the SM, the numbers of produced single top quarks and antiquarks are identical at the Tevatron. At the LHC, however, the initial state is not a eigenstate, and more top quarks than antiquarks are produced because in collisions the flux of up-type quarks is larger than the flux for down-type quarks.

The NLO QCD corrections for inclusive single top-quark production have been presented in Refs. Bordes:1994ki (); Stelzer:1997ns (); Stelzer:1998ni () for the -channel, in Ref. Smith:1996ij () for the -channel and in Refs. Giele:1995kr (); Zhu:2002uj () for the channel.

These cross sections are shown in table 2, assuming and using the MSTW2008lo/nlo68cl pdf set Martin:2009iq (). It turns out that the NLO corrections are only a few percent for the -channel and slightly larger for the channel. In contrast, the NLO corrections to the -channel contribution are about 30%. However, as has been pointed out before, this channel gives only a small contribution at the LHC. Since at NLO, no colour transfer between the two quark lines is allowed (the corresponding box contributions vanish after interference with the Born amplitude), it is conceivable that the small corrections are accidental and that the small scale uncertainty observed at NLO underestimates the possible size of the NNLO corrections. Very recently, the vertex corrections for the -channel have been calculated at NNLO QCD Brucherseifer:2014ama (). The corrections are found to be comparable in size to the NLO corrections.

Fully differential results at NLO accuracy for single top-quark production have been presented in Refs. Harris:2002md (); Sullivan:2004ie (); Sullivan:2005ar (). In Refs. Campbell:2004ch (); Cao:2004ky (); Cao:2005pq (); Campbell:2005bb (), the analysis has been extended by including the semileptonic decay of the top quark in the narrow-width approximation. In addition, the systematic combination of the NLO corrections with the parton shower has been investigated in MC@NLO Frixione:2005vw (); Frixione:2008yi () as well as in the Powheg framework Alioli:2009je (); Re:2010bp (). Beyond fixed-order perturbation theory, the impact of logarithmic corrections due to soft-gluon emission has been studied Mrenna:1997wp (); Kidonakis:2006bu (); Kidonakis:2007ej (); Kidonakis:2010ux (); Kidonakis:2010dk (); Kidonakis:2011wy ().

As will be seen below, the experimental study of single top-quark production is challenging—despite the sizeable cross sections—because of the complicated event signature and the large backgrounds. In contrast to production, singly-produced top quarks are highly polarised—a consequence of their coupling to the boson. The measurement of the top-quark polarisation thus provides a further test of the structure of the vertex. Assuming that the production mechanism is well understood, -channel single top-quark production can also be used to constrain the parton distribution in the proton. Furthermore, it can be used for a direct measurement of the CKM matrix element which is otherwise only indirectly accessible, via the assumptions of CKM matrix unitarity and of the existence of only three quark families.

### 6.1 t-Channel Production

Measurements of the -channel production cross section have been performed using events with exactly one isolated lepton (electron or muon) originating from the decay of the boson and two or three jets in the final state. One of the jets has to be identified as a jet. Additional requirements on kinematic observables, such as the missing transverse momentum or the transverse mass of the boson, are imposed in order to further remove background. Detailed and precise results are available from ATLAS and CMS Aad:2012ux (); Chatrchyan:2011vp (); Chatrchyan:2012ep (); Khachatryan:2014iya (); Aad:2014fwa ().

An early analysis of -channel single-top production was performed by the ATLAS collaboration based on an integrated luminosity of about  Aad:2012ux (). Events with two or three jets are selected. To separate -channel single top-quark signal events from backgrounds, several kinematic variables are combined into one discriminant by employing a neural network that also exploits correlations between the variables. The most discriminating variable for the two-jet sample is the invariant mass of the system formed by the -tagged jet, the charged lepton and the neutrino, , see figure 22(a). In the three-jet category, the invariant mass of the two leading jets and the absolute value of the difference in pseudo-rapidity of the leading and the lowest- jet are among the most discriminating variables. Multi-jet event yields are determined with data-driven techniques, while contributions from jets events are derived from simulation and normalised to data in control regions using a cut-based analysis. All other backgrounds and the -channel signal expectation are normalised to theoretical cross sections. To extract the signal content of the selected sample, a maximum-likelihood fit is performed to the output distributions of the neural net in the two-jet and three-jet data sets. From a simultaneous measurement in the two channels, a cross section of

 σt+¯t=83±4 (stat)+20−19 (% syst)pb

is measured. This result is confirmed in a cut-based analysis which is illustrated by the distribution in figure 22(b).

More recently, the CMS collaboration performed an analysis based on the full statistics available for  Khachatryan:2014iya (). The event sample is selected by the application of simple criteria: The events must contain exactly one muon or electron with large transverse momentum. They are categorised according to the numbers of jets and -tagged jets, and the category enriched with -channel signal is the one with two jets and one tag. One of the jets, denoted by , is expected to not originate from quarks, and its pseudo-rapidity distribution is typical of the -channel processes where a light parton recoils against a much more massive particle like the top quark. Signal events populate forward regions in the spectrum, and this feature is used to distinguish the signal from background. Background events from and from jets processes are determined by the use of control categories. In all categories the invariant mass is used to define a signal region and a side-band region that contain events inside and outside the reconstructed top-quark mass window of , respectively. To determine the contribution from signal events, a binned maximum-likelihood fit is performed to the distribution of the events in the signal region of the category with two jets and one tag. In figure 23 (a) the distribution is shown for events with forward jets. The figure illustrates that large-purity samples of -channel single-top quark events can be isolated at the LHC using simple selection criteria. The measured cross section for this process is