Hadronic topquark pairproduction with one jet
and parton showering
Abstract:
We present a calculation of heavyflavor production in hadronic collisions in association with one jet matched to parton shower Monte Carlo programs at nexttoleading order in perturbative QCD. Topquark decays are included and spin correlations in the decay products are taken into account. The calculation builds on existing results for the radiative corrections to heavyquark plus one jet production and uses the POWHEG BOX for the interface to the parton shower programs PYTHIA or HERWIG. A broad phenomenological study for the Large Hadron Collider and the Tevatron is presented. In particular we study—as one important sample application—the impact of the parton shower on the topquark charge asymmetry.
HUEP11/36
LPN1139
SFB/CPP1141
1 Introduction
The Large Hadron Collider (LHC) and the Tevatron provide a unique experimental environment for topquark physics. Already with the currently accumulated luminosity at both colliders, but even more so with the anticipated high statistics data in the LHC 7 TeV run, the prospects for precision studies of topquarks are excellent. Precise experimental measurements for topquark production demand theoretical predictions with comparable precision. Within Quantum Chromodynamics (QCD) this requires the knowledge of the hard scattering process beyond the leading order (LO) in perturbation theory. Predictions for the hadroproduction of topquark pairs, i.e., , are available at nexttoleading order (NLO) since long [1, 2, 3, 4], and can be improved further thanks to resummation or the use of approximate nexttonexttoleading order (NNLO) results, see e.g., [5, 6]. The NLO QCD corrections for the processes jet [7, 8] and jets [9, 10] are more recent achievements.
For the direct comparison with experimental data, however, e.g., in order to model experimental acceptances, it is important to provide also theory predictions for the production of fully exclusive events. Due to the inherent limitations of the fixedorder approaches, in the past these were simulated by shower Monte Carlo (SMC) programs, which were accurate to LO only. Nowadays, much better theoretical precision can be reached by merging NLO computations with parton showers. The merging method has been pioneered by MC@NLO [11]. As an attractive feature the approach combines the accuracy of exact hard matrix elements for the large angle scattering including the radiative corrections to first order in the strong coupling constant with the soft and collinear emission described by the parton shower. The former ingredient usually displays a reduced sensitivity with respect to variations of the renormalization and factorization scales and , while the latter accounts for the correct Sudakov suppression of collinear and soft emissions. The matching between the regions of hard and of soft and collinear emissions is smooth.
The followup development has seen an extension of the merging procedure by means of a method, dubbed POWHEG [12], which is independent of the parton SMC generator used. Moreover, the POWHEG method allows for the generation of positive weighted events only and thus for a very efficient event generation. The POWHEG BOX [13] now provides a general framework for implementing NLO calculations in SMC programs (see also [14] for progress towards further automation in MC@NLO). Processes involving the hadronic production of topquarks have been subject to these improvements from very early on. Topquark pairproduction and singletop production processes have been implemented in MC@NLO [15, 16] and POWHEG [17, 18, 19] since quite some time and are now widely used by experimental collaborations.
In this article, we are concerned with pairproduction in association with one hard jet, because a large fraction of inclusive events does actually contain one or even more additional jets. Moreover, due to the larger phase space, the relative importance of data samples with jets increases at the LHC with respect to the Tevatron. Topquark pairproduction associated with jets is also an important background to Higgs boson production in vector boson fusion and for many signals of new physics, e.g., those motivated by supersymmetry. For the process jet we are merging the NLO QCD corrections [7, 8] (see [20] for the impact of topquark decays) with the parton SMC HERWIG [21] and PYTHIA [22, 23] using the POWHEG BOX. An independent implementation of this process using the results of HELACNLO [9, 24] has been reported recently in ref. [25]. In this work we also include spincorrelation effects in the produced events.
The outline is a follows. In Sec. 2 we discuss the implementation details in the POWHEG BOX, which are specific to the process jet. We briefly describe the validation procedure and carefully examine details of the event generation in POWHEG. In Sec. 3 we present a phenomenological analysis for the Tevatron with TeV centerofmass energy (Sec. 3.1) and the LHC for TeV (Sec. 3.2). In case of the Tevatron we investigate the impact of the parton shower on the forwardbackward charge asymmetry which is currently measured at the Tevatron for the inclusive sample. For the LHC the impact on the charge asymmetry visible in the rapidity distribution is analyzed. Furthermore we discuss the inclusion of the topquark decay and its impact on differential distributions of the decay products. Our conclusions and our outlook on future developments are given in Sec. 4.
2 Implementation
The POWHEG BOX [13] provides a welldefined framework for implementing general NLO calculations in parton SMC programs. To that end, it requires as input particular information about the individual components of the NLO calculation under consideration, i.e., about the Born process, its virtual radiative corrections and the real emission contributions. Combination of the latter two and cancellation of the emerging soft and collinear singularities also requires the definition of a subtraction scheme. Within the POWHEG BOX the socalled FrixioneKunsztSigner (FKS) subtraction [26] is the method of choice.
For the reaction jet we are building on the computation of [7, 8] for the QCD corrections to NLO, which provides us with all necessary details. The list of all flavor structures of the partonic Born and the real emission processes can be obtained from generic matrix elements by considering all possible crossings of light particles into the initial state. In Born approximation these are given by
(1) 
and for the real corrections by
(2) 
with and .
We use MadGraph [27] for the computation of all Born squared amplitudes from eq. (1) and real emission matrix elements squared from eq. (2). Likewise, the color correlated Born squared amplitudes and the helicity correlated ones, both being necessary ingredients of NLO calculations employing a subtraction method, have been obtained by properly modifying the routines generated by MadGraph. Cross checks have been performed with AutoDipole [28]. Moreover, factorization in the soft and collinear limits has been explicitly checked in double and quadruple precision.
The finite part of the virtual corrections for jet is extracted from a C++ library of results [7, 8], which is compliant with the interface to parton SMC programs proposed in [29]. In brief, the virtual amplitudes and loop diagrams associated with eq. (1) are all generated analytically and, after manipulation with computer algebra programs, automatically translated into C++ code. The reduction of tensor integrals up to fivepoint functions displays good numerical stability. Finally, the calculation results in a decomposition of all loop diagrams according to helicity and color structure times scalar functions depending on the external momenta only. The infrared (IR)finite scalar integrals are evaluated using the FF package [30, 31] and an efficient caching system is applied to speedup the entire computation. The current implementation needs approximately 36 ms CPU time on an Intel Xeon processor with 3.00 GHz for each evaluation of the function (see eq. 4.5 of [13]) at a single phase space point, summing over all contributing subprocesses. About half of that time is spent on the computation of the virtual corrections.
[GeV]  [GeV]  [GeV]  [pb]  
TEV 1.96 TeV  
LHC 7 TeV  
LHC 14 TeV  
With the input described so far, our POWHEG BOX implementation can be used to generate hadronic events accurate to NLO. There is, however, an important technical issue related to multileg processes which are interfaced to a parton shower: Reactions such as parton possess soft and collinear divergences already at LO. Since the POWHEG method relies on generating all events starting from a momentum configuration of the underlying Born process, a generation cut, , needs to be placed on the transverse momentum of the finalstate partons, a procedure wellknown from standard SMC generators, see e.g., the discussion in [32].
This cut for the event generation, which in practice takes values e.g., GeV, is unphysical and has to be always much smaller than the analysis cut on the transverse momentum, , employed in the definition of the additional jet associated with the pair. The condition is necessary though not sufficient to provide a suitable sample of unweighted events, because the parton shower can in fact increase the transverse momentum in an event generated at Born level with a given . This may result in a different number of events that would have passed the analysis cut if the generation cut were different. Therefore, it is essential to show that the actual dependence on is negligible for a given fixed analysis cut . We have carefully investigated this issue, reporting some examples in Tab. 1, which shows the independence of the cross section on the generation cut for reasonable values of the cut. In particular, this is satisfied for smaller than . Tab. 1 provides also a strong cross check of existing results in [25].
Also a second option for dealing with processes with soft and collinear divergences at Born level is available by generating weighted rather than unweighted events and, thereby suppressing the divergences. The POWHEG BOX uses a suppressed cross section for the generation of the underlying Born configurations [32],
(3) 
where is a measure of the hardness of the extra emission, denotes the inclusive NLO cross section at fixed underlying Born variables (see eq. 4.2 of [13]), and has to be chosen such that it ensures finiteness of in the limit . Thus, becomes integrable and, of course, the generated events need to be weighted by . The POWHEG BOX implementation foresees the choice
(4) 
where the variable controls the extent of the suppression^{1}^{1}1 In the POWHEG BOX the value of can be assigned at run time trough the entry of the input card. and is process specific, for jet. In our event generation we have also applied the Born suppression factor of eq. (4) and checked its implementation for different values with very good numerical accuracy, as shown in Tab. 1.
2.1 Checks
The current implementation has been exposed to a large number of checks. These include, first of all, comparisons for a sizable number of differential distributions to NLO with the available fixed order results. We have used the settings of [7, 8], i.e., the renormalization and factorization scales GeV, the analysis cut of GeV and GeV for the Tevatron and LHC configuration, respectively, the parton distribution function (PDF) set CTEQ6M [33], the jet algorithm of [34] (inclusive) with and we have assumed here the topquarks to be always tagged and thus excluded from jet reconstruction. Perfect agreement with [7, 8] has been found typically at the permille level. Also note that the computation of [7, 8] has employed dipole subtraction with massive partons [35] for the cancellation of the soft and collinear divergences between the real and virtual contributions. As mentioned, the POWHEG BOX relies on FKS subtraction [26] and, of course, the results for physical cross sections at NLO must be independent of the chosen scheme, which constitutes another strong check of the current implementation.
The other aspect which demands careful checking is the parton shower. It adds allorder perturbative corrections, though to leading logarithmic accuracy only, and the POWHEG approach offers one particular choice of how these corrections beyond NLO are included. Since the merging with parton showers modifies the QCD predictions, sometimes even for inclusive quantities, one should check during the validation process that these modifications reflect real physics effects and moreover, are compatible with (un)known higherorder corrections. To that end, we have also compared the NLO fixed order and the POWHEG predictions after the first emission, i.e., at the level they are written to the Les Houches event file [36] (LHEF from now on), for suitable distributions in order to assess similarities and differences between the results. Of particular interest in this procedure are those observables, which display great sensitivity to the parton shower effects. Some results will be shown below in Sec. 3.
3 Results
Throughout this section we present our findings. In comparing to the fixed order NLO results we are using the parton shower programs HERWIG [21] (version 6.5.20) and PYTHIA [22, 23] (version 6.4.25), with the default setting of parameters. Moreover, in order to highlight the shower effects and to disentangle them from the underlying event (UE) or multiple particle interactions (MPI), we have generally switched off these features in the SMC programs. Of course MPI and UE, together with the usage of the appropriate SMC tuning, will play an important rôle when comparing POWHEG predictions with data. For the kind of study we are interested in, we have decided not to include them in the following plots and we have concentrated on presenting distributions which are not extremely sensitive to these effects, where possible. The one exception here is the discussion of the charge asymmetries, in Secs. 3.1.1 and 3.2.1. There, we will also consider the predictions obtained including also MPI and UE in our comparisons in order to asses the stability of our results with respect to these effects.
We have produced different samples of events, to study both, the Tevatron and LHC collider configurations. Each sample contains 20M positive and negative weighted events, produced without folding (see Appendix A) and with a generation cut GeV and GeV, respectively, for the Tevatron and the LHC. As already mentioned, the jet reconstruction cut in the analysis has been assumed to be GeV and GeV. We also make use of the option of the POWHEG BOX to damp the low transverse momentum regions in the cross section, artificially increasing the probability of a hard jet. For this reason, the events have a weight which is the inverse of eq. (4). The choices GeV for the Tevatron (LHC) were adopted.
For the sake of comparisons and, in order to keep the analysis routine rather insensitive to possible contamination in the jet reconstruction procedure, we always force the semileptonic decay of the (anti)topquark when interfacing to a SMC program in the following. Also, as already done for the NLO comparisons of Sec. 2, we will always use the jet algorithm of [34] (inclusive) with and the recombination scheme.^{2}^{2}2Comparisons have been done with other jet clustering algorithms, e.g., the anti jet algorithm [37] with scheme recombination, for different values of the parameter , without significantly changing the general conclusions drawn here. In addition, after interfacing to a SMC program and performing the hadronization stage, we always exclude from the jet list those jets which happen to contain a flavored hadron, whose origin can be traced back to the (anti)topquark decay.^{3}^{3}3This exclusion is applied also when the topquark decay is performed by POWHEG itself and bottomquarks coming from topquarks can be present already at the LHEF stage, as it will be the case in Sec 3.3. Other bottomquarks present at partonic level (or B hadron not originating from a (anti)topquark) are instead always consistently considered as (originating from) light partons and therefore included in the light jets count..
As we focus entirely on the effect of the parton SMC and the NLO merging, our phenomenological analysis in Secs. 3.1 and 3.2 follows [7, 8], fixes the renormalization and factorization scales GeV, and uses the PDF set CTEQ6M [33]. Studies of the theoretical uncertainty of the cross section for jet due to corrections of higher orders (beyond NLO in QCD) have already been conducted in [7, 8] with standard means, i.e., determining the variations for the scale choices of and . In Tab. 2 we report results for the Tevatron TeV as well as for the TeV and TeV LHC configurations allowing for the independent variations of and of factors and and, at the same time, excluding relative ratios of larger than or smaller than . We find a remarkable small variation, typically below 10% . On the basis of the scale variations uncertainty one can thus conclude that higher order effects should be small.
TEV TeV  

LHC TeV  
LHC TeV 
The other main source of theoretical uncertainties, related to the nonperturbative parameters such as the PDFs and the associated value of the strong coupling constant , have repeatedly been addressed in the literature (see e.g., [6]) using modern PDF sets available to NNLO [38, 39, 40]. For a more recent study concerning the combined uncertainty due to propagated PDF uncertainties and uncertainties in we refer the interested reader to the results discussed in [41]. The topquark mass is always taken as a pole mass, and we refer to [42] for a discussion of the running mass in the scheme.
3.1 Tevatron
We will begin our studies with the Tevatron ( TeV), which has provided us already with several measurements of differential distributions. These are, in detail, the first measurement of the cross section , differential in pair invariant mass , see [43], the dependence of the production cross section on the transverse momentum of the topquark [44] and most prominently, the measurements of the forwardbackward charge asymmetry in topquark pairproduction [45, 46] along with its dependence on the pair invariant mass [47, 48].
In all the plots throughout this article no acceptance cuts are imposed, other than those necessary to define the hard jet. The lines appearing the legenda are labeled according their origin: NLO for the fixed order computation, LHEF for the results after the POWHEG hardest emission without any showering and PWG+HER, PWG+PYT for the results obtained by generating the hardest emission with the POWHEG method and then performing the remaining shower and hadronization stages with the HERWIG or PYTHIA programs, respectively. The lower inset in each plot shows the relative difference with respect to the first entry in the legend, which is usually depicted as a solid black line in the upper inset. The black dots in the lower inset stand instead as a reference for the zero line. The Monte Carlo integration errors are shown as vertical bars.
In Fig. 1, we plot the differential cross section as a function of the transverse momentum of the topquark (upper panel) and of the the pair invariant mass (lower panel). A first comment can be made upon the expected good agreement between the NLO results and the LHEF ones for such inclusive quantities. The effect of the shower does not change considerably these results. Only at the very low and high ends we observe a significant change which is however still below 30%.
Similar conclusions can also be drawn looking at the upper panel of Fig. 2, where we plot the differential cross sections as a function of the azimuthal separation between the top and antitopquarks. In particular, this last observable is very stable with respect to the inclusion of the parton shower. With exception of the last bin, we observe corrections of a few percent only. The understanding is that the parton shower is not able to produce a significant change of the relative directions of the two outgoing heavy quarks. In the lower panel instead, we show the differential cross sections as a function of the transverse momentum of the pair. Shower effects at low values are now clearly visible. Furthermore, by inspecting the lower inset in the plot, showing the relative difference with NLO predictions, it is also possible to see a hint of the instabilities that may arise in the fixed order calculation around the GeV jet cut. This behaviour is easily explained considering that the region below the cut may be populated only when more than one hard jet is resolved, thus allowing for an imbalance between the hardest jet and the pair. Indeed, for the partons configuration, by momentum conservation. This effectively makes the distribution for lower than the jet cut a LO quantity, starting at . We have verified that the instability gets worse by reducing the bin size and that neither the LHEF nor the showered results show a similar behaviour. The same feature will also be present in LHC predictions, around the GeV jet cut, as we will show in the lower panel of Fig. 7. Such instabilities are well known to arise at any fixed order of the perturbative expansion whenever the observable under consideration has a nonsmooth behaviour inside the physical region or whenever the phase space boundary for a certain number of partons lies inside that for a larger number [49]. In our case the LO distribution is discontinuous at the jet boundary, since the phase space for partons does not allow , while it is different from zero at . It should be stressed that despite these effects are due to unbalanced cancellation of higher order soft/collinear divergences at the critical point(s), they are integrable in any finite neighborhood. In ref. [49] it was also demonstrated that the allorder resummation of soft divergences restores the infrared finiteness of the predictions also at the critical point by the appearance of continuous and infinitely differentiable structures, that were dubbed Sudakov shoulders. We have indeed verified that the resummation implicit in the POWHEG approach does reproduce these structures, as can be observed in the figures.
From Fig. 3 on we investigate the jet structure of the process. To that end, in Fig. 3, we display the differential cross sections (upper panel) and (lower panel) as function of the transverse momentum and rapidity of the hardest jet. Here we notice a moderate shape distortion and a different normalization in going from parton level to hadronic events. Both these effects can be understood by considering that the jet clustering procedure is significantly affected when going from a low multiplicity sample to a fully hadronized event. This is also reflected in the number of resolved jets above the minimum cut and in their kinematics.
In the upper panel of Fig. 4 we show the azimuthal difference between the hardest jet and the system. is very sensitive to shower effects, since at partonic level the hardest jet is constrained to reside in the opposite hemisphere w.r.t. the pair momentum. In the lower panel we plot the differential cross section as function of the transverse momentum of the system composed of the topquark, the antitopquark and the hardest jet. This observable is of particular importance, as it is strongly correlated with the transverse momentum of the nexttohardest jet. The latter, in turn, is the quantity where the Sudakov suppression effects should be most evident. Due to the jet reconstruction procedure, however, it turns out that those effects are best seen in the low region. The disagreement in the high tail between NLO and LHEF results, on the one side, and showered results, on the other, is instead due to showering and hadronization effects and is partly related to our choice of excluding the topquark from jet reconstruction. A similar effect has also been observed (and explained) in singletop production (see Sec. 4 of [50]) and we have verified that the same explanation can readily be applied here too, for the system: At high there exists an artificial imbalance due to many hadrons coming from the hardest parton which are not clustered together with the hardest jet. This creates an effective for the system containing the hardest jet, giving rise to the harder tail observed.
Finally, in Fig. 5 we plot the differential cross section as function of the transverse momentum and rapidity of the nexttohardest jet. No high enhancement, or suppression, is observed in this case. However, large differences in the normalization of distributions are present when going from NLO results to LHEF and showered ones. This can again be explained with the different number of configurations with are resolved by the reconstruction algorithm as containing two hard jets.
Tevatron TeV  NLO [%]  LHEF [%]  PWG+HER [%]  PWG+HER+UE [%]  PWG+PYT [%]  PWG+PYT+MPI [%] 

total  
total  
3.1.1 Topquark forwardbackward charge asymmetry
In view of the measurements of the forwardbackward asymmetry in topquark pairproduction at the Tevatron [45, 46, 47] we have also evaluated the values of the rapidity asymmetries in jet samples, at various stages of our simulations and with various acceptance cuts. The definitions for and used throughout this paper are
(5) 
where . Due to the fact that the initial state at the Tevatron is a CP eigenstate and due to the absence of CP violating effects in QCD, one has and corresponds to in the rest frame. When moving to the laboratory frame, where a greater accuracy can be reached on the experimental determination of these quantities, gets smaller in magnitude than , which in turn is a boostinvariant quantity, depending only on rapidity differences. We report both in Tab. 3, expressed as percentage values to ease their readability, at various stages of our simulation. We have also included the predictions obtained with the HERWIG and PYTHIA showers supplemented with underlyingevent and multiparton interactions activities, respectively, referring to them as PWG+HER+UE and PWG+PYT+MPI. In case of PWG+PYT+MPI the Perugia 0 Tune [51] – MSTP(5)=320 – has also been adopted.
For both asymmetries and shower models, we observe that the inclusion of the parton shower leads to a significant correction compared to the fixed order and LHEF predictions. For example, the results for total asymmetries are almost reduced by a factor of two by the partonshower. A similar effect is also observed in presence of selection cuts on the rapidity or invariant mass of the heavy quark pair. This outcome extends the conclusions obtained by previous combined NLO and parton shower simulations [47] for the inclusive sample.^{4}^{4}4 See also [52] for higherorder QCD corrections to and [10] for studies of the jet process in particular.
Inspecting the results shown in Tab. 3 more closely, we find that performing PYTHIA and HERWIG showers leads to similar predictions for : the values are fairly consistent once the statistical uncertainties are taken into account. The agreement is instead much worse for . The inclusion of underlyingevent or multiparticle interaction does not dramatically change this picture, the interleaved shower evolution due to MPI and Perugia 0 Tune in PYTHIA results in a larger difference with respect to the default behaviour than the simpler UE model in HERWIG.
The dependence of on the transverse momentum of the pair, , has also recently been reported in [48]. In ref. [53], the authors have investigated this behaviour in presence of selection cuts on the pair invariant mass, including also EW corrections. Since this observable only receives contributions starting at , even for the inclusive sample – an extra jet is always required to have a nonzero – our approach offers the possibility to evaluate it at NLO supplemented with shower effects for the first time. This should improve over the MC@NLO and POWHEG simulations for production, that are only leadingorder/leadinglogarithm accurate for when .
In Tab. 3 we have also included our predictions for the forwardbackward asymmetries with . We now see, that the results after showering with two different SMCs are consistent almost everywhere, apart from the very low region, which thus contributes to generate the differences in . Moreover, for both asymmetries and , we observe that for the inclusion of the partonshower leads to results in fair agreement with the NLO ones. The large differences between NLO and showered results observed in the total asymmetries are thus traced back to the region of small ’s. This appears plausible since in that region soft and collinear emission produced by the parton shower will be more important compared to the large region. We also note that our findings are different from the observations made in [48] where a stronger effect of the parton shower using specific tunes was observed over the entire range. One has to remind, however, that for a leadingorder SMC such as the PYTHIA program used in [48], the contributions to the asymmetry for are generated exclusively by the shower. It thus looks feasible that a change in the parton shower will be reflected in a overall change of the predictions.
Whether the aforementioned large corrections produced by the parton shower could be responsible in part for the observed discrepancy between theory and experiment is however unclear because in the sample this effect may cancel. Given the stability of the theoretical prediction above GeV —now available at NLO accuracy— a detailed comparison of experimental data and theory predictions may provide useful information to further scrutinize the observed discrepancy in the inclusive sample.
3.2 Lhc
In Figs. 6 to 11 we report a similar set of distributions as already shown for the Tevatron, this time for the LHC collider at TeV. For most of the observables, the same comments and conclusions as reported for the Tevatron case are, in general, valid here, too. For this reason, we will not repeat the same remarks here. There are, however, some new plots that deserve discussion and explanations.
In the lower panel of Fig. 6 we show the differential cross section as a function of the rapidity distribution of the topquark . This inclusive quantity shows the expected good agreement between NLO and LHEF results. It is also pretty stable with respect to the inclusion of parton shower effects, resulting only in a few percent change in the overall normalization.
In the upper panel of Fig. 9 we show the differential cross section as function of the scalar sum of the relative transverse momenta of the particles in the first jet, , which is defined with respect to the jet axis in the frame where the jet has zero rapidity. In general, we define for the th jet,
(6) 
where denotes the momentum of the particle in the th jet, see also [50]. The observable behaves as expected: The NLO curve shows the unphysical enhancement associated with the IR singularity at , the LHEF result corrects for this only partially, owing to the Sudakov suppression by finalstate radiation, while the fully showered events manifest the physical suppression at low . Moreover, in the lower panel of Fig. 9 we show the distribution of the invariant mass of the system made by the topquark and the hardest light jet.
Eventually, in the lower panel of Fig. 10, the total exclusive cross section as a function of the number of resolved jets, , is shown. The moderate difference in the bin between the NLO and LHEF results may be considered a consequence of the different normalization of the distributions involving the nexttohardest jet, as shown e.g., in Fig. 11. Higher bins are instead populated only by the shower and thus predictions for those bins are only accurate in the strict soft/collinear limit.
One noticeable difference w.r.t. Tevatron results is the reduced discrepancy between the showered and partonic results for observables that involve the hardest or nexttohardest jets, e.g., Figs. 8 and 11. A possible explanation for this is in the higher jet cut ( GeV) used for LHC analysis, that largely restricts the regions where shower effects may become important.
A first phenomenological application of the POWHEG implementation discussed here has already been reported in [54], namely the study of events at the LHC as a function of the invariant mass of the multijet systems as a means of measuring the topquark mass.
LHC TeV  NLO [%]  LHEF [%]  PWG+HER [%]  PWG+HER+UE [%]  PWG+PYT[%]  PWG+PYT+MPI [%] 

Tevatron TeV  LHEF [%]  PWG+HER [%]  PWG+HER+UE [%]  PWG+PYT [%]  PWG+PYT+MPI [%] 

PWG+HER’ [%]  PWG+HER’+UE [%]  PWG+PYT’ [%]  PWG+PYT’+MPI[%]  
3.2.1 Topquark charge asymmetry
In Tab. 5 we present our estimate of the charge asymmetries in the sample, measured with respect to the (anti) topquark pseudorapidity and rapidity , at various stages of our simulation. The two observables are defined in the same way
(7) 
with and or ,
respectively. By looking at our results, one can see that a positive
asymmetry is present for both observables, albeit larger in magnitude
for . Moreover, results obtained with the inclusion of
PYTHIA and HERWIG showers are in fair agreement, even after the
addition of MPI or UE. We also observe that the numerical evaluation
of the asymmetry is rather challenging at fixed order, leading to
large statistical uncertainties. Only after increasing the statistics
by one order of magnitude we were able to obtain errors comparable
with those obtained after the inclusion of the parton shower. We
consider the results including the effects of the parton shower as the
best prediction currently available for the asymmetry. We refer to
refs. [55, 56] for recent LHC
measurements of and in the inclusive
sample.
In closing we remark, that we have also carefully tested the LHC nominal centerofmass energy, producing the same set of distributions as in Figs. 6 to 11 for TeV collisions. Since no significant difference in the behaviour has been observed in any of the distributions, with respect to the TeV case, we refrain from including the corresponding plots here.
3.3 Topquark decay
The studies so far have been based on the assumption of stable (anti)topquarks during both the fixed order calculation stage and the generation of the hardest radiation according to the POWHEG method. Thus, the output resulting from these stages includes onshell topquarks and extra light partons only. When interfacing to a SMC program for performing the rest of the showering and the hadronization steps, no information concerning the spin or helicity of these topquarks is retained and the decay is performed by the SMC, which averages over the possible top polarizations.
In this way one does not correctly account for topquark offshell effects, nonresonant production mechanisms and for the topquark spin correlations. However, given the large ratio between the topquark mass and the topquark width, the first two effects are suppressed as and, therefore, are rather modest. This was also explicitly shown for the production case by the recent calculation of the NLO corrections to the final state [57, 58].
Topquark spin correlations at hadron colliders were instead realized to be an important tool to study topquark properties since the early work of [59]. Also, the QCD corrected spin analyzing power of jets in decays of polarized topquarks has been extensively discussed in [60]. The possibility to measure these correlation effects is particular to topquarks because of their large mass and short lifetime, which prevent nonperturbative QCD effects from significantly depolarizing them before the decay.
The usual approach to study this phenomenon relies on taking the topquark zerowidth limit and separately considering NLO corrections to the production and decay processes. This is done by means of a spin correlation matrix which accounts for all the possible spin configurations occurring in the two stages. Several studies following this approach have already been presented, concerning both production [59] with spin correlations at NLO and the case [20] with spin correlations accounted for at leading order.
Here we follow a different approach, that was first introduced in [61] and has already been employed and discussed in both implementations, POWHEG [18, 19, 62] and MC@NLO [16, 63]. In this way we avoid having to introduce the spin correlation matrices, but we nevertheless recover the exact leadingorder spin correlations. To be more precise, we have LO spincorrelations in the soft and collinear regions, while the same accuracy of the complete NLO calculation, namely the matrix element,
(8) 
is used for the hard regions.^{5}^{5}5In case no radiation harder than GeV is generated by the POWHEG method, the event is classified as Bornlike: the corresponding matrix elements for the decayed process , i.e., , are then employed. For the sake of brevity, we explain this method here only briefly, and instead, refer to the aforementioned publications for more details. The basic idea is to first generate events with stable topquarks (undecayed events) through the usual POWHEG machinery and then generate the decay products according to the matrix element for the full production and decay process (decayed events).
Moreover, in order to produce more realistic final states, we have also allowed for a reshuffling of the momenta of the topquark decay products, resulting in offshell topquarks and bosons, whose virtualities have been distributed according to BreitWigner shapes. This reshuffling is such that the relative 3momentum of the (anti)topquark in the rest frame and the 3momentum of the radiated light partons in the partonic centerofmass system are kept fixed. It also takes care of the small changes in the phase space and luminosity due to the and quark being slightly offshell with respect to the chosen pole mass value. In any case, we restrict the topquark and virtualities offshellness to be in between widths. We have checked that this modification does not significantly change the results obtained in the topquark and boson zerowidth approximation, by comparing several distributions for the two cases.^{6}^{6}6 The zerowidth approximation in the decay may always be enforced by setting the zerowidth token to 1 in the input card.
Furthermore, since charged leptons (or downtype quarks) coming from the topquark decays are the most sensitive probe of the topquark spin directions, we concentrate on the dileptons channel only. We thus always assume and , with branching ratio . However, we stress that our implementation is completely general for what concerns the topquark decay products, such that the lepton+jets or the all hadronic search channels can be simulated as well, if desired.^{7}^{7}7See e.g., [64] for a review of observables sensitive to spincorrelation effects in the lepton+jets channel.
Thus, taking as an example the semileptonic topquark decay channel, the conditional probability for the decayed events, starting from undecayed ones, is obtained from
(9) 
where is the full space phase including the decay products, while ’s are the matrix elements squared for the given partonic process. In practice, however, to generate configurations according to eq. (9), one makes use of an upper bound for the ratio and then proceed as follows:

Generate a tentative decay kinematics , starting from .

Extract a random value in the range .

If , then the decay kinematics is allowed and the event is accepted. Otherwise go back to step I.
An efficient functional form of the upperbounding function may be readily reconstructed from the structure of topquarks decay:
(10) 
where and are the topquark and W boson virtualities and and are the squared amplitudes for the decay processes. The choice of the normalization factor has been performed by sampling the allowed phase space, by requiring that the inequality
(11) 
always holds, for any given specific subprocess flavour .
In the rest of this section we present results obtained within this approach. We have set
(12) 
and we have considered a simplified form for the CKM matrix, with a mixing between the first two generations only:
(13) 
and all the other entries set to zero. No extra acceptance cuts on the leptons are placed in the following plots.
With these ingredients we are able to offer predictions for topquarks decay products, at the LHEF level and after shower and hadronization. We compare them in Fig. 12 , where we plot the positively charged lepton transverse momentum and the rapidity of the negatively charged one, at the LHC and Tevatron colliders, respectively. We note that in these distributions shower effects are rather small. Moreover, one does not expect to see any dependence on the topquark spin.
Spin correlation effects in production are usually studied by choosing and spin quantization axis and looking at reference frames and angular distributions that are particularly sensitive to these correlations^{8}^{8}8See e.g., [65] for strategies to maximize the spin correlation of pairs produced at the LHC., a procedure that can easily be performed in SMC simulations. However, due to the presence of unobserved neutrinos, this can become a difficult task in the data analysis for an experimental collaboration. An example of such observables is the double differential distribution,
(14) 
where and are the angles between the directions of the flights of the leptons coming from the decayed topquark in the () rest frame and an arbitrary direction that defines the quantization axis for the (anti)topquark spin.
The double differential distribution in eq. (14) can be evaluated to good approximation to
(15) 
which is only valid, though, for fully inclusive cross sections. As soon as cuts are imposed the form of the distribution will change and a further dependence on could be introduced.^{9}^{9}9We note that electroweak effects and QCD absorptive parts lead to a tiny polarization of the topquark and thus a deviation from the simple form in eq. (15) of the double differential distribution shown in eq. (14), even in the absence of cuts. The cuts may also affect the simple interpretation of , which in general depends also on the choice of the spin quantization axis. Nevertheless even in the presence of cuts the distribution is still a useful observable to study the impact of spin correlations. This quantity has been recently measured by D0 [66] for the choice of the beam direction as quantization axis, finding . Due to the large uncertainties, this value is both compatible with no spin correlation and with the NLO predictions of [59].
In Fig. 13 we present our predictions for the distribution in eq. (14) at the Tevatron using the beamaxis to define the lepton angles, obtained by including the spin correlation effects as explained above in our sample. We compare these results with those obtained by letting the SMC program performing the uncorrelated topquark decays. The effect of the spin correlations is clearly visible, leading to differences as large as at extreme values.
Alternatively, one can look at the distributions of the topquark decay products in the laboratory frame. In this case the problem is to devise clever enough cuts to single out spincorrelation effects which are usually hardly visible.^{10}^{10}10 A recent paper [67] suggests the use of these distributions to construct a likelihood function for the spincorrelation hypothesis, that can be then tested statistically for its validity. See also [68, 69] for uptodate results using this approach at Tevatron.
There are, however, notable exceptions. One such example, the azimuthal distance between the leptons coming from the top and the antitopquark, has already been shown in [70] to depend mildly on spincorrelations. Results for this observable has also been presented in [71], for the ongoing LHC TeV run. Later on, it has been suggested that imposing the acceptance cut should enhance this dependence in the dilepton search channel at the LHC [64]. However, due to the inherent ambiguities of the unobserved neutrinos, the true value cannot be reconstructed on an eventbyevent basis in a real experiment. In our case, we simply looked back in the shower history to reconstruct unambiguously the true . A more realistic study would use the definition of value averaged over all the possible neutrino assignments proposed by the authors of [64]. However, as shown in [64], this only leads to minor differences.
In Fig. 14 we show our results with both the HERWIG and PYTHIA showers and the hadronization stage simulations. In both panels, spin correlation effects are again clearly visible as a change in the slope of the distribution.
As a final remark, we investigate the effects induced by topquark charge asymmetries on the dilepton final state, by studying the leptonic charge asymmetries. This issue has also been addressed in a recent paper [72], for the inclusive production, including nexttoleading order QCD and EW corrections. In ref. [20], the authors provide predictions for this quantity at NLO in the sample. The definitions for the asymmetries follow the ones in eq. (5), but are expressed in term of leptonic rapidities in the laboratory frame:
(16) 
with . We present our results in Tab. 5, also reporting, for ease of comparisons, the results including UE and MPI and the ones for the uncorrelated case, which we dub PWG+HER’ and PWG+PYT’, where the (anti)topquark decay is performed by the SMC neglecting spincorrelation effects . Comparing the results including the spin correlation to the results where the topquark decay is handled by the shower program — spin correlations are thus not taken into account in the latter predictions— we observe only a small difference between the two approaches. On the other hand a significant change can be observed when comparing LHEF results with the results including shower effects. Our conclusion is that most of the effect present at parton level is washed out by the parton shower. Indeed, investigating the behaviour of the leptonic forwardbackward charge asymmetries in presence of a cut on the transverse momentum of the intermediate pair, one can trace back the large differences between results at partonic and hadronic level to the region of low ’s once again, as it was the case for the topquark forwardbackward charge asymmetry shown in Tab. 3.
4 Conclusions
We have studied topquark hadroproduction in association with a jet merged with parton showers to NLO in QCD. For that purpose, we have presented an implementation of the process jet in the framework of POWHEG BOX. A careful validation has been performed by comparing with known results. For Tevatron and LHC at