../Common/references.bib \AtlasTitleSearch for Minimal Supersymmetric Standard Model Higgs bosons and for a boson in the final state produced in collisions at TeV with the ATLAS Detector \AtlasRefCodeHIGG-2015-08 \PreprintIdNumberCERN-EP-2016-164 \AtlasJournalRefEur. Phys. J. C76 (2016) 585 \AtlasDOI10.1140/epjc/s10052-016-4400-6 \AtlasJournalEur. Phys. J. C. \AtlasAbstractA search for neutral Higgs bosons of the Minimal Supersymmetric Standard Model (MSSM) and for a heavy neutral boson is performed using a data sample corresponding to an integrated luminosity of 3.2 fb from proton–proton collisions at \TeV recorded by the ATLAS detector at the LHC. The heavy resonance is assumed to decay to a pair with at least one lepton decaying to final states with hadrons and a neutrino. The search is performed in the mass range of 0.2–1.2 \TeV for the MSSM neutral Higgs bosons and 0.5–2.5 \TeV for the heavy neutral boson. The data are in good agreement with the background predicted by the Standard Model. The results are interpreted in MSSM and benchmark scenarios. The most stringent constraints on the MSSM – space exclude at 95% confidence level (CL) for \GeV in the MSSM scenario. For the Sequential Standard Model, a mass up to 1.90 \TeV is excluded at 95% CL and masses up to 1.82–2.17 \TeV are excluded for a of the Strong Flavour Model.
- 1 Introduction
- 2 Data sample and Monte Carlo simulation
- 3 Object reconstruction and identification
- 4 Search channels
- 5 Background estimation
- 6 Systematic uncertainties
- 7 Results
- 8 Conclusions
The discovery of a scalar particle at the LHC [ATLASHiggsJuly2012, CMSHiggsJuly2012] has provided important insight into the mechanism of electroweak symmetry breaking. Experimental studies of the new particle [Aad:2015mxa, Aad:2015gba, Khachatryan:2014jba, Khachatryan:2014kca, ATLAS-CONF-2015-044] demonstrate consistency with the Standard Model (SM) Higgs boson [ENGLERT, HIGGS, HIGGS2, HIGGS3, Guralnik:1964eu, Kibble:1967sv]. However, it remains possible that the discovered particle is part of an extended scalar sector, a scenario that is favoured by a number of theoretical arguments [Djouadi:2005gj, Branco:2011iw].
The Minimal Supersymmetric Standard Model (MSSM) [Fayet:1976et, Fayet:1977yc, Farrar:1978xj, Fayet:1979sa, Dimopoulos:1981zb] is the simplest extension of the SM that includes
supersymmetry. The MSSM requires two Higgs doublets of opposite hypercharge. Assuming that CP symmetry is
conserved, this results in one CP-odd () and two CP-even (, ) neutral Higgs bosons and two
charged Higgs bosons (). At tree level, the properties of the Higgs sector in the MSSM depend on only
two non-SM parameters, which can be chosen to be the mass of the CP-odd Higgs boson, , and the
ratio of the vacuum expectation values of the two doublets, . Beyond tree level,
additional parameters affect the Higgs sector, the choice of which defines
various MSSM benchmark scenarios. In some scenarios, such as [MSSMBenchmarks],
the top-squark mixing parameter is chosen such that
the mass of the lightest CP-even Higgs boson, , is close to the measured mass of the Higgs
boson that was discovered at the LHC.
A different approach is employed in the hMSSM scenario [Djouadi:2013uqa, Bagnaschi:2015hka] in which
the value of can be used, with certain assumptions, to predict the remaining masses and couplings of the MSSM Higgs bosons without explicit reference to the soft supersymmetry-breaking parameters.
The couplings of the MSSM heavy Higgs bosons to down-type fermions are enhanced with respect to the
SM for large values, resulting in increased branching fractions to leptons and
Heavy \Zprime gauge bosons appear in several models [Hewett:1989, Cvetic:1995zs, Leike:1998wr, Rizzo:2006nw, Diener:2010sy] and are a common extension of the SM [Langacker:2008]. Such \Zprime bosons can appear in theories extending the electroweak gauge group, where lepton universality is typically conserved. A frequently used benchmark is the Sequential Standard Model (SSM) [SSM], which contains a single additional \Zprime boson with the same couplings as the SM boson. Some models offering an explanation for the high mass of the top-quark, predict instead that such bosons couple preferentially to third-generation fermions [ZprimeToThirdGen, sfm, G221, TopFlavor]. A model predicting additional weak gauge bosons \Zprime and \Wprime coupling preferentially to third-generation fermions is the Strong Flavour Model (SFM) [sfm, TopFlavor].
Direct searches for high-mass resonances decaying to have been performed by the ATLAS [ATLASZprime5fb] and CMS [CMSZprime5fb] collaborations using 5
2 Data sample and Monte Carlo simulation
The ATLAS detector [ATLASDetector] at the LHC consists of an inner tracking detector with a
coverage in pseudorapidity
Simulated events with a heavy neutral MSSM Higgs boson produced via gluon–gluon fusion and in association with -quarks are generated with the POWHEG-BOX v2 [Nason:2004rx, Frixione:2007vw, Powheg3] and MADGRAPH5_aMC@NLO 2.1.2 [Alwall:2014hca, Wiesemann:2014ioa] programs, respectively. The CT10 [Lai:2010vv] and CT10nlo_nf4 [Dulat:2015mca] sets of parton distribution functions (PDFs) are used, respectively. PYTHIA 8.210 [PYTHIA82] with the AZNLO [AZNLO:2014] (A14 [ATL-PHYS-PUB-2014-021]) set of tuned parameters, or “tune”, is used for the parton shower, underlying event and hadronization in the gluon–gluon fusion (-associated) production. The production cross sections for the various MSSM scenarios are calculated using SusHi [Harlander:2012pb] for gluon fusion production [Harlander:2002wh, Spira:1995rr, Anastasiou:2002yz, Ravindran:2003um, Harlander:2002vv, Anastasiou:2002wq, Aglietti:2004nj, Bonciani:2010ms, Harlander:2004tp, Harlander:2005rq, Degrassi:2010eu, Degrassi:2011vq, Degrassi:2012vt] and -associated production in the five-flavour scheme [Harlander:2003ai]; -associated production in the four-flavour scheme is calculated according to Refs. [Dittmaier:2003ej, Dawson:2004a]. The final -associated production cross section is obtained by using the method in Ref. [SantanderMatching] to match the four-flavour and five-flavour scheme cross sections. The masses and the couplings of the Higgs bosons are computed with FeynHiggs [Heinemeyer:1998yj, Heinemeyer:1998np, Frank:2006yh, Degrassi:2002fi, Hahn:2013ria], whereas the branching fraction calculation follows the procedure described in Ref. [Heinemeyer:2013tqa]. In the case of the hMSSM scenario, the procedure described in Ref. [Bagnaschi:2015hka] is followed for the production cross sections and HDECAY [Djouadi:1997yw] is used for the branching fraction calculation.
The signals are simulated by reweighting a leading-order (LO) \DY sample using the TauSpinner algorithm [Czyczula:2012ny, Kaczmarska:2014eoa, TauSpinnerBSM] to account for spin effects in the decays. The \DY sample, enriched with high invariant mass events, is generated with PYTHIA 8.165 [Pythia8] using the NNPDF2.3LO PDF set [Ball:2012cx] and the A14 tune for the underlying event. Interference between the \Zprime signals and the SM \DYonly production is not included.
The simulated backgrounds consist of the production of +jets, +jets, pairs, single top quarks and electroweak dibosons (). These are modelled with several event generators as described below, while contributions from multi-jet production are estimated with data as described in Section 5.
Simulated samples of +jets events for the and channels and +jets events for the channel are produced using POWHEG-BOX v2 interfaced to PYTHIA 8.186 with the AZNLO tune. In this sample, PHOTOS++ v3.52 [photos, Davidson:2010ew] is used for final-state QED radiation. A dedicated +jets sample binned in , produced using the SHERPA 2.1.1 generator [Gleisberg:2008ta], is used in the channel in order to enhance the number of events with high invariant mass. For this sample, matrix elements are calculated for up to two partons at next-to-leading order (NLO) and four partons at LO, merged with the SHERPA parton shower model using the ME+PS@NLO prescription [Hoeche:2012yf]. Spin correlation effects between the boson and its decay products are simulated with the TauSpinner program. All /+jets samples use the CT10 PDF set and are normalized to the next-to-next-to-leading-order (NNLO) cross sections calculated using FEWZ [Anastasiou:2003ds, Melnikov:2006kv, Gavin:2010az].
The POWHEG-BOX v2 program with the CT10 PDF set is used for the generation of pairs and single top quarks in the - and -channels. Samples of -channel single-top-quark events are produced with the POWHEG-BOX v1 generator employing the four-flavour scheme for the NLO matrix element calculations together with the fixed four-flavour scheme PDF set CT10f4; the top-quark decay is simulated with MadSpin [Artoisenet:2012st]. For all samples of top-quark production, the spin correlations are preserved and the parton shower, fragmentation and underlying event are simulated using PYTHIA 6.428 [Pythia] with the CTQ6L1 PDF set and the corresponding Perugia 2012 tune [Skands:2010ak]. Final-state QED radiation is simulated using PHOTOS++ v3.52. The top-quark mass is set to 172.5 \GeV. The production sample is normalized to the NNLO cross section, including soft-gluon resummation to next-to-next-to-leading-logarithm accuracy (Ref. [Czakon:2011xx] and references therein). The normalization of the single-top-quark event samples uses an approximate NNLO calculation from Refs. [Kidonakis:2011wy, Kidonakis:2010tc, Kidonakis:2010ux].
Finally, diboson processes are simulated using the SHERPA 2.1.1 program with the CT10 PDF. They are calculated for up to one additional parton at NLO, depending on the process, and up to three additional partons at LO. The diboson samples use the NLO cross sections SHERPA calculates.
The simulation of - and -hadron decays for all samples, excluding those generated with SHERPA, uses EvtGen v1.2.0 [evtgen]. All simulated samples include the effect of multiple proton-proton interactions in the same and neighbouring bunch crossings (“pile-up”) by overlaying simulated minimum-bias events on each generated signal or background event. These minimum-bias events are generated with PYTHIA 8.186 [Pythia, Pythia8], using the A2 tune [ATLAS:2012uec] and the MSTW2008LO PDF [Martin:2009iq]. Each sample is simulated using the full GEANT4 [Geant4, ATLASSIM] simulation of the ATLAS detector, with the exception of the -associated MSSM Higgs boson signal, for which the ATLFAST-II [ATLASSIM, ATLAS:1300517] fast simulation framework is used. Finally, the Monte Carlo (MC) samples are processed through the same reconstruction software as for the data.
3 Object reconstruction and identification
The primary vertex of each event is chosen as the protonâproton vertex candidate with the highest sum of the squared transverse momenta of all associated tracks. Electron candidates are reconstructed from energy deposits in the electromagnetic calorimeter associated with a charged-particle track measured in the inner detector. The final electron candidates are required to pass the “loose” likelihood-based identification selection [Aad:2014nim, ATLAS-CONF-2016-024], to have a transverse energy and to be in the fiducial volume of the inner detector, . The transition region between the barrel and end-cap calorimeters () is excluded.
Muon candidates are reconstructed from track segments in the muon spectrometer, matched with tracks found in the inner detector within . The tracks of the final muon candidates are refit using the complete track information from both detector systems and are required to have a transverse momentum and to pass the “loose” muon identification requirements [ATLASRun2Muon].
Both the electrons and muons are required to pass a -dependent isolation selection, which utilizes both calorimetric and tracking information, with an efficiency of 90% (99%) for transverse momentum of . The isolation provides an efficiency that grows as a function of lepton , since the background from jets faking leptons becomes less important as the lepton increases. The contributions from pile-up and the underlying event activity are corrected on an event-by-event basis using the ambient energy density technique [IsolationPileUp1].
Jets are reconstructed from topological clusters [Aad:2016upy] in the calorimeter using the anti- algorithm [AntiKT], with a radius parameter value . To reduce the effect of pile-up, a jet vertex tagger algorithm is used for jets with and . It employs a multivariate technique based on jet energy, vertexing and tracking variables to determine the likelihood that the jet originates from pile-up [ATLASJVT]. In order to identify jets containing -hadrons (-jets), a multivariate algorithm is used [ATL-PHYS-PUB-2015-022, ATL-PHYS-PUB-2015-039]. A working point that corresponds to an average efficiency of 70% for -jets in simulated events is chosen. The misidentification rates for -jets, -jets and jets initiated by light quarks or gluons for the same working point and in the same sample of simulated events are approximately 10%, 4% and 0.2% respectively.
Hadronic decays of leptons are predominantly characterized by the presence of one or three charged particles, accompanied by a neutrino and possibly neutral pions. The reconstruction of the visible decay products, hereafter referred to as , starts with jets with . The candidate must have energy deposits in the calorimeters in the range , with the transition region between the barrel and end-cap calorimeters excluded. Additionally, they must have , one or three associated tracks and an electric charge of . A multivariate boosted decision tree (BDT) identification, based on calorimetric shower shape and track multiplicity of the candidates, is used to reject backgrounds from jets. In this analysis, two identification criteria are used: “loose” and “medium” with efficiencies measured in decays of about 60% (50%) and 55% (40%) for one-track (three-track) candidates, respectively [ATLAS:tauperfrun2]. An additional dedicated likelihood-based veto is used to reduce the number of electrons misidentified as .
Signals in the detector can be used in more than one reconstructed object. Objects that have a geometric overlap are removed according to the following priorities:
Jets within a cone around a selected are excluded.
Jets within a cone around an electron or muon are excluded.
Any within a cone around an electron or muon is excluded.
Electrons within a = 0.2 cone around a muon are excluded.
The missing transverse momentum () is calculated as the modulus of the negative vectorial sum of the of all fully reconstructed and calibrated jets and leptons [ATL-PHYS-PUB-2015-027]. This procedure includes a “soft term”, which is calculated based on the inner-detector tracks originating from the primary vertex that are not associated to reconstructed objects.
4 Search channels
Events in the channel are recorded using single-muon triggers and a logical-OR combination of single-electron triggers. Single-electron triggers with thresholds of , and are used for the channel. For the channel, a single-muon trigger with a threshold of is used if the muon is larger than and a single-muon trigger with a threshold of is used otherwise. The triggers impose electron and muon quality requirements which are tighter for the triggers with lower thresholds.
Events must have at least one identified candidate and either one electron or one muon candidate which is geometrically matched to the HLT object that triggered the event. Events with more than one electron or muon fulfilling the criteria described in Section 3 are rejected in order to reduce the backgrounds from production, where ,. The selected lepton must have a transverse momentum and pass the “medium” identification requirement.
The candidate is required to have , pass the “medium” BDT-based identification requirement and lie in the range . The latter requirement is motivated by a larger rate of electrons misidentified as candidates at higher values: the rate is above 10% for , while it ranges from 0.5% to 3% for lower values. If there is more than one candidate, the candidate with the highest is selected and the others are treated as jets. Finally, the identified lepton and the are required to have opposite electric charge.
Subsequently, the following selection requirements are applied:
For the channel, events are vetoed if the invariant mass of the electron and the visible lepton decay products is in the range .
The requirement on gives an overall reduction of SM backgrounds with little signal loss. The requirement on , the distribution of which is shown in Figure 2(a), serves to remove events that originate from processes containing a boson: in signal events, the missing transverse momentum is usually in the same direction as the , resulting in a low value of . The requirement on reduces the contribution of decays, where an electron is misidentified as a candidate. These selection criteria define the inclusive selection.
Events in the channel are selected by a trigger that requires a single satisfying the “medium” identification criterion with . The leading candidate in must geometrically match the HLT object. A requirement is applied to the leading candidate, , and to the sub-leading candidate, . Furthermore, the leading (sub-leading) candidate has to satisfy the “medium” (“loose”) identification criterion. Events with electrons or muons fulfilling the loose selection criteria described in Section 3 (with the exception of the isolation requirement) are vetoed to reduce electroweak background processes and guarantee orthogonality with the channel.
The leading and sub-leading candidates must have opposite electric charge and have a back-to-back topology in the transverse plane, . The distribution of before this requirement is shown in Figure 2(b). This selection defines the inclusive selection.
4.3 Event categories
In the search for \Zprime bosons, the event selections described in
Sections 4.1 and 4.2 result in a signal selection
-veto: no -tag jets in the event,
-tag: at least one -tag jet in the event.
In the \bveto category, the signal selection efficiency varies between 2% at and 7% at for the gluon–gluon fusion production mode in the channel, and from 0.1% to 15% in the channel for the same mass range. In the \btag category, the signal selection efficiency varies from 0.5% at to 2% at for the -associated production mode in the channel, and from 0.1% to 6% in the channel.
4.4 Di-tau mass reconstruction
The di-tau mass reconstruction is critical in achieving good separation between signal and background. However, its reconstruction is challenging due to the presence of neutrinos from the lepton decays. The mass reconstruction used for both the and channels is the total transverse mass, defined as
where is defined as
and refers to the visible decay of the lepton ( or ). More complex mass reconstruction techniques were investigated, but they did not improve the expected sensitivity.
5 Background estimation
The background processes can be categorized according to whether the electron/muon and/or the are correctly identified. Backgrounds from processes with correctly identified , electrons and muons, or where the is due to a misidentified electron/muon in the channel, are estimated from simulation. Data-driven techniques are used for processes where the , or both the lepton and are misidentified. The background contributions originating from processes where only the lepton is misidentified are found to be negligible.
|signal region||, ,|
|Veto for ,|
|(-tag category), (-veto category) or|
|no requirement ( category)|
|+jets fake factor control region||70 (60) \GeV for (),|
|different identification for anti- sub-region|
|Multi-jet fake factor control region||invert isolation requirement,|
|different identification for anti- sub-region|
|Multi-jet control region for||30 \GeV, no isolation requirement,|
|estimation||no passing loose identification,|
|(-veto category), (-tag category)|
|Control region for correction of electrons||for 1-track|
|misidentified as||for 3-track|
|(-tag category), (-veto category) or|
|no requirement ( category)|
|Multi-jet fake factor control region||pass single-jet trigger, leading fails medium identification,|
|no tracks, nor charge requirements for leading ,|
|, no requirement|
|Fake-rate control region||pass single-muon trigger, isolated muon with ,|
|with , ,|
|(for -veto category only)|
|\Wmunu control region for||pass single-muon trigger, isolated muon with ,|
|+jets \MT correction||with|
5.1 background estimate
The main backgrounds in the channel arise from production, followed by processes with a misidentified in the -veto category and production, with either a true lepton or a jet misidentified as a , in the -tag category.
Background processes where the candidate, or both the lepton and candidates, arise from misidentified jets are dominated by +jets () and multi-jet processes, for the -veto (-tag) category. A data-driven “fake factor” (FF) technique is used to estimate the contribution of these processes to the signal region. The fake factors are derived separately for the -veto and -tag categories using fake factor control regions (see Table 1) dominated by a particular background process (Pr), and are defined as:
where is the number of candidates in data satisfying the “medium” identification criterion and is the number of candidates failing this criterion but meeting a loose requirement on the BDT score. The latter requirement defines the “anti-” sub-region, which selects the same kind of objects mimicking candidates as those fulfilling the identification criteria. The true contamination in the fake factor control regions is subtracted using simulation. In all the control regions, the fake factors are parameterized as a function of the transverse momentum and number of tracks of the reconstructed object.
The fake factor for +jets and backgrounds, FF+jets, is measured in a fake factor control region that is identical to the signal region, except that the selection criterion is reversed to for the () channel. The purity of the +jets background in the -veto category of the control region is about , while in the -tag category both the +jets and processes contribute. The fake factor value for the -tag category was found to be compatible with the value corresponding to the -veto category. To improve the statistical precision, the fake factor measured in a control region without requirements on the number of -tags is used for the -tag category. The same fake factor is used in the search for the \Zprime boson. For multi-jet events (MJ), the fake factor FF is measured in a fake factor control region defined by inverting the isolation requirement on the electron or muon. The purity of multi-jet events in this control region exceeds %. The fake factors are derived separately for the -veto and -tag categories by requiring no -tag and at least one -tag, respectively. For the analysis, no -tag requirement is considered.
The shapes and normalization of background contributions in the signal region are then estimated by applying these fake factors to events that pass the anti- region selection but otherwise satisfy all signal region requirements. In this analysis, the fake factors are combined and weighted by the predicted contribution of each background process to the anti- region:
where denotes the fraction of multi-jet events in the anti- region and . This neglects the differences between the fake factors for +jets/ and other processes, such as production. The parameter is estimated, separately for the -veto and -tag categories, in two steps using a data-driven method. First, the rates at which jets are misidentified as electrons or muons are measured from the ratio of leptons passing and failing the lepton isolation requirement in a region enriched in multi-jet events. This multi-jet control region is defined in Table 1. The predicted multi-jet rate is then applied to events in the anti- sub-region that also fail the lepton isolation, in order to calculate as a function of separately for the and channels. When the fake factor is applied to the anti- sub-region events, the contributions from correctly identified \tauhadvis and from electrons and muons misidentified as \tauhadvis candidates are subtracted using the default MC simulation described in Section 2.
Background processes where the electron or the muon is identified as a object are modelled using simulation. The main source of such backgrounds is +jets events in the channel, which are reduced using the mass-window veto described in Section 4.1. To account for mismodelling of electrons misidentified as objects in +jets events, the simulation is corrected as a function of the lepton using data control regions defined by reversing the mass-window criterion, as listed in Table 1. The correction amounts to 15% for three-track , while for the one-track objects the correction varies from 20% in the barrel region to up to 200% in the end-cap region.
5.2 background estimate
The dominant background process for the channel is multi-jet production, the cross section of which is several orders of magnitude higher than that of the signal processes. Despite the large suppression of this background thanks to the event selection, a sizeable contribution of events with two jets misidentified as candidates remains. A fake factor technique is used to normalize and model this background. Fake factors parameterized as a function of and the number of tracks are derived from a control region enriched with multi-jet events, described in Table 1. The factors are derived independently for the -tag and -veto categories in the search for bosons, and inclusively in the search for \Zprime bosons. They are then applied to data events where the leading has passed the identification requirement in the signal region, while the sub-leading candidate has passed only a loose requirement on the BDT score. The contributions from non-multi-jet production processes are subtracted using simulation.
For and +jets events, along with other simulated background processes, the probability of a jet being misidentified as a is modelled with a “fake-rate” technique. The rates of jets being misidentified as a are measured from data as a function of the transverse momentum and number of tracks of the reconstructed \tauhadvis. The fake-rate control regions are described in Table 1 and are enriched in +jets for the -veto category and events for the -tag category,
The fake rate is then applied to the simulated events as a weight for each of the reconstructed that does not match geometrically a true lepton. Fake rates derived in the fake-rate control region of the -tag category are used for simulated and single top quark events, while fake rates obtained in the -veto control region are applied to the remaining processes. An additional weight is applied to +jets events as a function of \MT, to improve the modelling of the kinematics of the +jets simulated events. The reweighting function is derived by fitting the ratio of the data to the simulation for the process in an additional \Wmunu control region, defined in analogy with the inclusive signal selection and described in Table 1.
A same-sign validation region, enriched with events where at least one jet is misidentified as a \tauhadvis, is obtained by inverting the opposite-sign requirement of the two candidates. Distributions of in the channel same-sign validation region are shown in Figures 3(c) and 3(d). The good performance multi-jet background estimation method is demonstrated by the agreement of the data with the background prediction.
6 Systematic uncertainties
The signal efficiency and the background estimates are affected by uncertainties associated with the detector simulation, the signal modelling and the data-driven background determination.
The integrated luminosity measurement has an uncertainty of and is used for all MC samples. Uncertainties related to the detector are included for all signal and backgrounds that are estimated using simulated samples. These uncertainties are also taken into account for simulated samples that are used in the derivation of data-driven background estimates. All instrumental systematic uncertainties arising from the reconstruction, identification and energy scale of candidates, electrons, muons, (-)jets and the soft term of the \met measurement are considered. The effect of the energy scale uncertainties on the objects is propagated to the \met determination. The electron, muon, jet and systematic uncertainties described above are found to have a very small effect.
Systematic uncertainties resulting from the data-driven background estimates are derived as follows. In the channel, the combined fake-factor method includes uncertainties in the +jets fake factors, the multi-jet fake factors, and the estimation. For the +jets fake factors the main uncertainties arise from the dependence on , from the difference between the relative contributions of quark- and gluon-initiated jets faking in the control region and the signal region, and from the contamination by backgrounds other than +jets in the control region, which are estimated using simulation. The uncertainty is parameterized as a function of the anti- \pt and amounts approximately to for jets misidentified as one-track candidates and varies between 16% and 34% for jets misidentified as three-track candidates. Uncertainties related to non-+jets events were studied and have no significant impact on the fake-factor determination. For the multi-jet fake factors and , the uncertainty is dominated by the number of data events in the control region and the subtraction of the remaining non-multi-jet backgrounds using simulation. Typical values of the total uncertainties for are between 7% and 20% and for the multi-jet fake factors between 10% and 20%, depending on the channel and the candidate . In addition, the effect on the background estimate due to the anti- region definition is examined. The loose identification requirement used in the definition of this region is varied to estimate the corresponding uncertainty, which is and in the and the channel, respectively.
In the channel, the uncertainty in the fake-factor measurement used for the multi-jet background estimation is obtained as the sum in quadrature of the statistical uncertainty of the measurement and the difference between the fake factors determined from same-sign and from opposite-sign events. The fake rates for jets misidentified as are determined from data. The main systematic uncertainty arises from the statistical uncertainty of the fake-rate measurement and it ranges from 7% to 30% as a function of the . In the channel, the uncertainty in the parameters of the function used to reweight the +jets background is propagated to the \MT distribution, where its effect ranges from 5% to 20%.
Theoretical cross-section uncertainties are considered for all backgrounds estimated using simulation. For +jets and diboson production, uncertainties of and are used, respectively, combining PDF and scale variation uncertainties in quadrature. For [Czakon:2011xx] and single top-quark [Aliev:2010zk, Kant:2014oha] production, a uncertainty is assigned based on scale, PDF and top-quark mass uncertainties. Additional uncertainties related to initial- and final-state radiation modelling, tune and (for only) the choice of the hdamp parameter value in POWHEG-BOX v2, which controls the amount of radiation produced by the parton shower, were also taken into account [ATLAS:TopMCsyst]. The uncertainty in the fragmentation model is evaluated by comparing events generated with POWHEG-BOX v2 interfaced to either HERWIG++ [Herwigpp] or PYTHIA6. The POWHEG+HERWIG++ and aMC@NLO+HERWIG++ generators are used to estimate the uncertainty in generating the hard scatter. The variation of the -tag category acceptance for these uncertainties is from to ( to ) in the () channel.
Uncertainties related to signal modelling are discussed in the following. Uncertainties due to the factorization and renormalization scale choices are estimated from the effect on the signal acceptance of doubling or halving these factors either coherently or oppositely. Uncertainties due to the initial- and final-state radiation, as well as multiple parton interaction for the signal are also taken into account. These uncertainties are estimated from the PYTHIA8 A14 tune [ATL-PHYS-PUB-2014-021] for the -associated production and the AZNLO PYTHIA8 tune [AZNLO:2014] for the gluon–gluon fusion production. The envelope of the variations resulting from the use of the alternative PDFs in the PDF4LHC15nlo100 [Ball:2014uwa] set is used in order to estimate the PDF uncertainty for gluon–gluon fusion production. For the -associated production uncertainty, a comparison among NNPDF30_nlo_as_0118_nf_4 [Ball:2014uwa], CT14nlo_NF4 [Dulat:2015mca], MSTW2008nlo68cl_nf4 [Martin:2010db] and CT10_nlo_nf4 [Lai:2010vv] PDF sets is employed. Since no statistically significant effect on the shape of the reconstructed mass distribution is observed, each contribution is taken solely as a normalization uncertainty. The total uncertainty ranges between and .
The parameter of interest is the signal strength, . It is defined as the ratio of the observed to the predicted value of the cross section times branching fraction, where the prediction is evaluated for a particular MSSM or assumption. Hence, the value corresponds to the absence of a signal, whereas the value indicates the presence of a signal as predicted by the theoretical model under study. To estimate , a likelihood function constructed as the product of Poisson probability terms is used. Signal and background predictions depend on systematic uncertainties, which are parameterized as nuisance parameters and are constrained using Gaussian probability distributions. For the MSSM Higgs boson search a binned likelihood function is constructed in bins of the distributions, chosen to ensure sufficient background statistics in each bin. The search for a \Zprime boson is a counting experiment, summing the number of events above a certain \mttot threshold. The threshold is chosen for each \Zprime mass hypothesis to maximize the expected significance and ranges from 400 \GeV at low \Zprime mass to 750 \GeV at high \Zprime mass. The asymptotic approximation is used with the test statistic [Cowan:2010js] to test the compatibility of the data with the assumed signal.
The number of observed and data events, along with the predicted event yields from background and signal processes, in the signal regions are shown in Table 2. The observed event yields are compatible with the expected event yield from SM processes, within uncertainties. The mass distributions are shown in Figure 4. The results from the and channels are combined to improve the sensitivity to and \Zprime boson production.
|-tag category||-veto category|
|and single top quark||115||16||35||5|
|-tag category||-veto category|
|and single top quark||136||15||40||5|
|-tag category||-veto category|
|and single top quark||11||3||4.5||0.9|
The fractional contributions of the most important sources of systematic uncertainty to the total uncertainty in the signal cross-section measurement are shown for two signal assumptions: Table 3(top) represents an MSSM Higgs boson hypothesis ( \GeV, ) and Table 3(bottom) corresponds to an SSM \Zprime boson hypothesis ( \TeV). As shown in this table, the sensitivity of the search is limited by statistical uncertainties.
|Source of uncertainty||(%)||(%)|
|and single-top-quark backgrounds normalization|
|\tauhadvis energy scale|
|Jet-to- fake rate ()|
|Multi-jet background ()|
|Jet-to- fake rate ()|
|Statistics (data and simulation)|
|Source of uncertainty||(%)||(%)|
|\tauhadvis energy scale|
|jets backgrounds cross section and acceptance|
|Jet-to- fake rate ()|
|+jets background reweighting ()|
|Statistics (data and simulation)|
The data are found to be in good agreement with the predicted background yields and hence the results are given as exclusion limits. These are set using the modified frequentist method known as CL [CLs_2002]. Observed and expected 95% confidence level (CL) upper limits on the cross section times branching fraction for the production of a single scalar boson decaying to , as a function of the mass of the boson , are shown in Figures 5(a) and 5(b). The limits are calculated for both the gluon–gluon fusion and -associated production modes, using a combination of the and channels and assuming the natural width of the boson to be negligible compared to the experimental resolution (as expected over the probed MSSM parameter space). The lowest excluded cross section times branching fraction values range from at to at for a scalar boson produced via gluon–gluon fusion. Similarly, for the -associated production mechanism the lowest excluded values range is from at to at .
The observed and expected 95% CL limits on as a function of , for the combination of and channels in the MSSM and hMSSM scenarios are shown in Figures 5(c) and 5(d). The expected limit in the scenario is compared to the expected limits from the individual and channels. For the figure, lines of constant and are shown. For the hMSSM scenario, the exclusion arising from the SM Higgs boson coupling measurements of Ref. [Aad:2015pla] is also shown, in addition to the ATLAS Run-1 search result of Ref. [Aad:2014vgg]. The constraints in the hMSSM scenario are stronger than those in the scenario. This is due to the presence of low-mass neutralinos in the scenario that reduce the branching fraction and which are absent in the hMSSM scenario. In the hMSSM scenario, the most stringent constraints on for the combined search exclude for and for at the 95% CL. In the MSSM scenario, the 95% CL upper limits exclude for and for . The feature of the expected limits in the hMSSM scenario exclusion plot at around \GeV is due to the behaviour of the branching ratio close to the kinematic threshold. Some sensitivity of the search is also expected around , \GeV due to the increase of the gluon–gluon fusion cross section induced by the increased coupling to the top quark.
In the search for the \Zprime boson, the observed number of events in the signal regions of the and channels are consistent with the SM predictions. The resulting 95% CL upper limits are set on the cross section times branching fraction as a function of the mass and shown in Figure 6(a). These results are interpreted in the context of the SSM and SFM in Figures 6(a) and 6(b), respectively. The resulting observed (expected) lower limit on the mass of the \ZPSSM boson is () \TeV. In the search for the \ZprimeSFM boson, results are presented as a function of , where is the mixing angle between the two SU(2) gauge eigenstates of the model. Masses below \ZPSFMLOWESTLIMIT–\ZPSFMHIGHESTLIMIT \TeV are excluded in the range , assuming no mixing. For the value of , the lower limit on the mass of a \ZprimeSFM boson is \ZPSFMLIMITLOWSINSQUAREPHI \TeV, extending the limits from previous direct and indirect searches by more than 200 \GeV.
A search for neutral Higgs bosons of the Minimal Supersymmetric Standard Model (MSSM) and for a \Zprime gauge boson decaying to a pair of leptons is performed using a data sample corresponding to an integrated luminosity of \currentlumirange from proton–proton collisions at \TeV recorded by the ATLAS detector at the LHC. The search finds no indication of an excess over the expected background in the channels considered. Limits are set at the 95% CL, which provide constraints in the MSSM parameter space. Model-independent upper limits on the production cross section times the branching fraction of a scalar boson versus its mass, in both the gluon–gluon fusion and -associated production modes, are presented. The upper limits on the cross section times branching fraction range from at to at for a scalar boson produced via gluon–gluon fusion (-associated production). In the context of the MSSM scenario, the most stringent 95% CL upper limit on for the combined search is for . This analysis extends the limits of the previous searches for the mass range . The search for a \Zprime boson is interpreted in the context of the Sequential Standard Model (SSM) and the Strong Flavour Model (SFM). Upper limits at the 95% CL are set on the cross section times branching fraction as a function of the \Zprime mass. The observed lower limit on the \Zprime mass is \TeV for a \ZPSSM and ranges from \ZPSFMLOWESTLIMIT to \ZPSFMHIGHESTLIMIT \TeV as a function of the parameter for a \ZprimeSFM.
We thank CERN for the very successful operation of the LHC, as well as the support staff from our institutions without whom ATLAS could not be operated efficiently.
We acknowledge the support of ANPCyT, Argentina; YerPhI, Armenia; ARC, Australia; BMWFW and FWF, Austria; ANAS, Azerbaijan; SSTC, Belarus; CNPq and FAPESP, Brazil; NSERC, NRC and CFI, Canada; CERN; CONICYT, Chile; CAS, MOST and NSFC, China; COLCIENCIAS, Colombia; MSMT CR, MPO CR and VSC CR, Czech Republic; DNRF and DNSRC, Denmark; IN2P3-CNRS, CEA-DSM/IRFU, France; GNSF, Georgia; BMBF, HGF, and MPG, Germany; GSRT, Greece; RGC, Hong Kong SAR, China; ISF, I-CORE and Benoziyo Center, Israel; INFN, Italy; MEXT and JSPS, Japan; CNRST, Morocco; FOM and NWO, Netherlands; RCN, Norway; MNiSW and NCN, Poland; FCT, Portugal; MNE/IFA, Romania; MES of Russia and NRC KI, Russian Federation; JINR; MESTD, Serbia; MSSR, Slovakia; ARRS and MIZŠ, Slovenia; DST/NRF, South Africa; MINECO, Spain; SRC and Wallenberg Foundation, Sweden; SERI, SNSF and Cantons of Bern and Geneva, Switzerland; MOST, Taiwan; TAEK, Turkey; STFC, United Kingdom; DOE and NSF, United States of America. In addition, individual groups and members have received support from BCKDF, the Canada Council, CANARIE, CRC, Compute Canada, FQRNT, and the Ontario Innovation Trust, Canada; EPLANET, ERC, FP7, Horizon 2020 and Marie Skłodowska-Curie Actions, European Union; Investissements d’Avenir Labex and Idex, ANR, Région Auvergne and Fondation Partager le Savoir, France; DFG and AvH Foundation, Germany; Herakleitos, Thales and Aristeia programmes co-financed by EU-ESF and the Greek NSRF; BSF, GIF and Minerva, Israel; BRF, Norway; Generalitat de Catalunya, Generalitat Valenciana, Spain; the Royal Society and Leverhulme Trust, United Kingdom.
The crucial computing support from all WLCG partners is acknowledged gratefully, in particular from CERN, the ATLAS Tier-1 facilities at TRIUMF (Canada), NDGF (Denmark, Norway, Sweden), CC-IN2P3 (France), KIT/GridKA (Germany), INFN-CNAF (Italy), NL-T1 (Netherlands), PIC (Spain), ASGC (Taiwan), RAL (UK) and BNL (USA), the Tier-2 facilities worldwide and large non-WLCG resource providers. Major contributors of computing resources are listed in Ref. [ATL-GEN-PUB-2016-002].
The ATLAS Collaboration
M. Aaboud, G. Aad, B. Abbott, J. Abdallah, O. Abdinov, B. Abeloos, R. Aben, O.S. AbouZeid, N.L. Abraham, H. Abramowicz, H. Abreu, R. Abreu, Y. Abulaiti, B.S. Acharya, S. Adachi, L. Adamczyk, D.L. Adams, J. Adelman, S. Adomeit, T. Adye, A.A. Affolder, T. Agatonovic-Jovin, J. Agricola, J.A. Aguilar-Saavedra, S.P. Ahlen, F. Ahmadov, G. Aielli, H. Akerstedt, T.P.A. Åkesson, A.V. Akimov, G.L. Alberghi, J. Albert, S. Albrand, M.J. Alconada Verzini, M. Aleksa, I.N. Aleksandrov, C. Alexa, G. Alexander, T. Alexopoulos, M. Alhroob, B. Ali, M. Aliev, G. Alimonti, J. Alison, S.P. Alkire, B.M.M. Allbrooke, B.W. Allen, P.P. Allport, A. Aloisio, A. Alonso, F. Alonso, C. Alpigiani, A.A. Alshehri, M. Alstaty, B. Alvarez Gonzalez, D. Álvarez Piqueras, M.G. Alviggi, B.T. Amadio, K. Amako, Y. Amaral Coutinho, C. Amelung, D. Amidei, S.P. Amor Dos Santos, A. Amorim, S. Amoroso, G. Amundsen, C. Anastopoulos, L.S. Ancu, N. Andari, T. Andeen, C.F. Anders, G. Anders, J.K. Anders, K.J. Anderson, A. Andreazza, V. Andrei, S. Angelidakis, I. Angelozzi, P. Anger, A. Angerami, F. Anghinolfi, A.V. Anisenkov, N. Anjos, A. Annovi, C. Antel, M. Antonelli, A. Antonov, F. Anulli, M. Aoki, L. Aperio Bella, G. Arabidze, Y. Arai, J.P. Araque, A.T.H. Arce, F.A. Arduh, J-F. Arguin, S. Argyropoulos, M. Arik, A.J. Armbruster, L.J. Armitage, O. Arnaez, H. Arnold, M. Arratia, O. Arslan, A. Artamonov, G. Artoni, S. Artz, S. Asai, N. Asbah, A. Ashkenazi, B. Åsman, L. Asquith, K. Assamagan, R. Astalos, M. Atkinson, N.B. Atlay, K. Augsten, G. Avolio, B. Axen, M.K. Ayoub, G. Azuelos, M.A. Baak, A.E. Baas, M.J. Baca, H. Bachacou, K. Bachas, M. Backes, M. Backhaus, P. Bagiacchi, P. Bagnaia, Y. Bai, J.T. Baines, O.K. Baker, E.M. Baldin, P. Balek, T. Balestri, F. Balli, W.K. Balunas, E. Banas, Sw. Banerjee, A.A.E. Bannoura, L. Barak, E.L. Barberio, D. Barberis, M. Barbero, T. Barillari, M-S Barisits, T. Barklow, N. Barlow, S.L. Barnes, B.M. Barnett, R.M. Barnett, Z. Barnovska-Blenessy, A. Baroncelli, G. Barone, A.J. Barr, L. Barranco Navarro, F. Barreiro, J. Barreiro Guimarães da Costa, R. Bartoldus, A.E. Barton, P. Bartos, A. Basalaev, A. Bassalat, R.L. Bates, S.J. Batista, J.R. Batley, M. Battaglia, M. Bauce, F. Bauer, H.S. Bawa, J.B. Beacham, M.D. Beattie, T. Beau, P.H. Beauchemin, P. Bechtle, H.P. Beck, K. Becker, M. Becker, M. Beckingham, C. Becot, A.J. Beddall, A. Beddall, V.A. Bednyakov, M. Bedognetti, C.P. Bee, L.J. Beemster, T.A. Beermann, M. Begel, J.K. Behr, C. Belanger-Champagne, A.S. Bell, G. Bella, L. Bellagamba, A. Bellerive, M. Bellomo, K. Belotskiy, O. Beltramello, N.L. Belyaev, O. Benary, D. Benchekroun, M. Bender, K. Bendtz, N. Benekos, Y. Benhammou, E. Benhar Noccioli, J. Benitez, D.P. Benjamin, J.R. Bensinger, S. Bentvelsen, L. Beresford, M. Beretta, D. Berge, E. Bergeaas Kuutmann, N. Berger, J. Beringer, S. Berlendis, N.R. Bernard, C. Bernius, F.U. Bernlochner, T. Berry, P. Berta, C. Bertella, G. Bertoli, F. Bertolucci, I.A. Bertram, C. Bertsche, D. Bertsche, G.J. Besjes, O. Bessidskaia Bylund, M. Bessner, N. Besson, C. Betancourt, A. Bethani, S. Bethke, A.J. Bevan, R.M. Bianchi, L. Bianchini, M. Bianco, O. Biebel, D. Biedermann, R. Bielski, N.V. Biesuz, M. Biglietti, J. Bilbao De Mendizabal, T.R.V. Billoud, H. Bilokon, M. Bindi, S. Binet, A. Bingul, C. Bini, S. Biondi, T. Bisanz, D.M. Bjergaard, C.W. Black, J.E. Black, K.M. Black, D. Blackburn, R.E. Blair, J.-B. Blanchard, T. Blazek, I. Bloch, C. Blocker, A. Blue, W. Blum, U. Blumenschein, S. Blunier, G.J. Bobbink, V.S. Bobrovnikov, S.S. Bocchetta, A. Bocci, C. Bock, M. Boehler, D. Boerner, J.A. Bogaerts, D. Bogavac, A.G. Bogdanchikov, C. Bohm, V. Boisvert, P. Bokan, T. Bold, A.S. Boldyrev, M. Bomben, M. Bona, M. Boonekamp, A. Borisov, G. Borissov, J. Bortfeldt, D. Bortoletto, V. Bortolotto, K. Bos, D. Boscherini, M. Bosman, J.D. Bossio Sola, J. Boudreau, J. Bouffard, E.V. Bouhova-Thacker, D. Boumediene, C. Bourdarios, S.K. Boutle, A. Boveia, J. Boyd, I.R. Boyko, J. Bracinik, A. Brandt, G. Brandt, O. Brandt, U. Bratzler, B. Brau, J.E. Brau, W.D. Breaden Madden, K. Brendlinger, A.J. Brennan, L. Brenner, R. Brenner, S. Bressler, T.M. Bristow, D. Britton, D. Britzger, F.M. Brochu, I. Brock, R. Brock, G. Brooijmans, T. Brooks, W.K. Brooks, J. Brosamer, E. Brost, J.H Broughton, P.A. Bruckman de Renstrom, D. Bruncko, R. Bruneliere, A. Bruni, G. Bruni, L.S. Bruni, BH Brunt, M. Bruschi, N. Bruscino, P. Bryant, L. Bryngemark, T. Buanes, Q. Buat, P. Buchholz, A.G. Buckley