Measurement of spin correlation between top and antitop quarks produced in pp̄ collisions at √ s = 1 . 96 TeV D 0 Collaboration

V.M. Abazov af, B. Abbott bp, B.S. Acharya z, M. Adams au, T. Adams as, J.P. Agnew ap, G.D. Alexeev af, G. Alkhazov aj, A. Alton be,2, A. Askew as, S. Atkins bc, K. Augsten g, V. Aushev am, Y. Aushev am, C. Avila e, F. Badaud j, L. Bagby at, B. Baldin at, D.V. Bandurin bw, S. Banerjee z, E. Barberis bd, P. Baringer bb, J.F. Bartlett at, U. Bassler o, V. Bazterra au, A. Bean bb, M. Begalli b, L. Bellantoni at, S.B. Beri x, G. Bernardi n, R. Bernhard t, I. Bertram an, M. Besançon o, R. Beuselinck ao, P.C. Bhat at, S. Bhatia bg, V. Bhatnagar x, G. Blazey av, S. Blessing as, K. Bloom bh, A. Boehnlein at, D. Boline bm, E.E. Boos ah, G. Borissov an, M. Borysova am,13, A. Brandt bt, O. Brandt u, R. Brock bf, A. Bross at, D. Brown n, X.B. Bu at, M. Buehler at, V. Buescher v, V. Bunichev ah, S. Burdin an,3, C.P. Buszello al, E. Camacho-Pérez ac, B.C.K. Casey at, H. Castilla-Valdez ac, S. Caughron bf, S. Chakrabarti bm, K.M. Chan az, A. Chandra bv, E. Chapon o, G. Chen bb, S.W. Cho ab, S. Choi ab, B. Choudhary y, S. Cihangir at, D. Claes bh, J. Clutter bb, M. Cooke at,12, W.E. Cooper at, M. Corcoran bv, F. Couderc o, M.-C. Cousinou l, J. Cuth v, D. Cutts bs, A. Das bu, G. Davies ao, S.J. de Jong ad,ae, E. De La Cruz-Burelo ac, F. Déliot o, R. Demina bl, D. Denisov at, S.P. Denisov ai, S. Desai at, C. Deterre ap,4, K. DeVaughan bh, H.T. Diehl at, M. Diesburg at, P.F. Ding ap, A. Dominguez bh, A. Dubey y, L.V. Dudko ah, A. Duperrin l, S. Dutt x, M. Eads av, D. Edmunds bf, J. Ellison ar, V.D. Elvira at, Y. Enari n, H. Evans ax, A. Evdokimov au, V.N. Evdokimov ai, A. Fauré o, L. Feng av, T. Ferbel bl, F. Fiedler v, F. Filthaut ad,ae, W. Fisher bf, H.E. Fisk at, M. Fortner av, H. Fox an, J. Franc g, S. Fuess at, P.H. Garbincius at, A. Garcia-Bellido bl, J.A. García-González ac, V. Gavrilov ag, W. Geng l,bf, C.E. Gerber au, Y. Gershtein bi, G. Ginther at, O. Gogota am, G. Golovanov af, P.D. Grannis bm, S. Greder p, H. Greenlee at, G. Grenier q,r, Ph. Gris j, J.-F. Grivaz m, A. Grohsjean o,4, S. Grünendahl at, M.W. Grünewald aa, T. Guillemin m, G. Gutierrez at, P. Gutierrez bp, J. Haley bq, L. Han d, K. Harder ap, A. Harel bl, J.M. Hauptman ba, J. Hays ao, T. Head ap, T. Hebbeker s, D. Hedin av, H. Hegab bq, A.P. Heinson ar, U. Heintz bs, C. Hensel a, I. Heredia-De La Cruz ac,5, K. Herner at, G. Hesketh ap,7, M.D. Hildreth az, R. Hirosky bw, T. Hoang as, J.D. Hobbs bm, B. Hoeneisen i, J. Hogan bv, M. Hohlfeld v, J.L. Holzbauer bg, I. Howley bt, Z. Hubacek g,o, V. Hynek g, I. Iashvili bk, Y. Ilchenko bu, R. Illingworth at, A.S. Ito at, S. Jabeen at,14, M. Jaffré m, A. Jayasinghe bp, M.S. Jeong ab, R. Jesik ao, P. Jiang d,‡, K. Johns aq, E. Johnson bf, M. Johnson at, A. Jonckheere at, P. Jonsson ao, J. Joshi ar, A.W. Jung at,16, A. Juste ak, E. Kajfasz l, O. Karacheban am, D. Karmanov ah, I. Katsanos bh, M. Kaur x, R. Kehoe bu, S. Kermiche l, N. Khalatyan at, A. Khanov bq, A. Kharchilava bk, Y.N. Kharzheev af, I. Kiselevich ag, J.M. Kohli x, A.V. Kozelov ai, J. Kraus bg, A. Kumar bk, A. Kupco h, T. Kurča q,r, V.A. Kuzmin ah, S. Lammers ax, P. Lebrun q,r, H.S. Lee ab, S.W. Lee ba, W.M. Lee at, X. Lei aq, J. Lellouch n, D. Li n, H. Li bw, L. Li ar, Q.Z. Li at, J.K. Lim ab, D. Lincoln at, J. Linnemann bf, V.V. Lipaev ai, R. Lipton at, H. Liu bu, Y. Liu d, A. Lobodenko aj, M. Lokajicek h,


Introduction
The top quark is the heaviest elementary particle in the standard model (SM) [1][2][3][4]. Despite the fact that the top quark decays weakly, its large mass leads to a very short lifetime of ≈ 5 · 10 −25 s [5][6][7]. It decays to a W boson and a b quark before hadronizing, a process that has a characteristic time of 1/ QCD ≈ (200 MeV) −1 equivalent to τ had ≈ 3.3 · 10 −24 s, where QCD is the fundamental scale of quantum chromodynamics (QCD). The top quark lifetime is also smaller than the spin-decorrelation time from spin-spin interactions with the light quarks generated in the fragmentation process [8], τ spin ≈ m t / 2 QCD ≈ (0.2 MeV) −1 ≈ 3 · 10 −21 s [9]. The top quark thus provides a unique opportunity to measure spin-related phenomena in the quark sector by exploiting kinematic properties of its decay products.
In proton-antiproton (pp) collisions, the dominant process for producing top quarks is through top-antitop ( tt ) quark pairs. This QCD process yields unpolarized t and t quarks, but leaves the spins of t and t correlated. A spin correlation observable can be defined as [10] O ab = 4(S t ·â)(S¯t ·b) = σ (↑↑) + σ (↓↓) − σ (↑↓) − σ (↓↑) σ (↑↑) + σ (↓↓) + σ (↑↓) + σ (↓↑) , where S is a spin operator, â, b are the spin quantization axes for the top quark (â) and the antitop quark (b), refers to an expectation value, σ is the tt production cross section, and the arrows refer to the spin states of the t and t quarks relative to the â and b axes. The strength of the correlation depends on the tt production mechanism [11][12][13]. In pp collisions at a center-ofmass energy of 1.96 TeV, the correlation of spins is predicted to be O off = 0.80 +0.01 −0.02 [10] in the off-diagonal spin basis, the basis in which the strength of the spin correlation is maximal at the Tevatron [12]. The most significant contribution is from the quark-antiquark annihilation process (qq → tt) with a spin correlation strength of ≈ 0.99, while the gluon-gluon (gg) fusion process (gg → tt) has anticorrelated spins with a typical strength of ≈ −0.36 at next-to-leading order (NLO) in QCD [10,14,15]. Contributions to tt production from beyond the SM can have different dynamics that affect the strength of the tt spin correlation.
Evidence for tt spin correlations based on a matrix element technique [16], was presented by the D0 collaboration. Earlier lower precision measurements used a template method [17,18]. Spin correlation effects have also been measured in proton-proton (pp) collisions by two LHC collaborations, ATLAS and CMS, at a center-of-mass energy of 7 TeV [19][20][21][22] and at 8 TeV [23,24]. The main mechanism for tt production at the LHC is the gg fusion process. The spin correlation at the LHC arises mainly from the fusion of like-helicity gluons [25]. The differences between pp and pp incident channels, the different sources of spin correlation (quarkantiquark annihilation versus like-helicity gg fusion), and their different collision energies, make the measurements of the strength of the spin correlation at both the Tevatron and LHC interesting and complementary.
In this letter, we present an updated measurement of the tt spin correlation strength in pp collisions at √ s = 1.96 TeV. The measurement uses the statistics accumulated during 2001-2011 data taking period of the Fermilab Tevatron Collider, which corresponds to an integrated luminosity of 9.7 fb −1 , which is almost two times more than in our previous publication [16].

Detector, event selection and simulation, background
The D0 detector is described in Refs. [26][27][28][29][30][31][32]. It has a central tracking system consisting of a silicon microstrip tracker and a central fiber tracker, both located within an ∼ 2 T superconducting solenoidal magnet. The central tracking system is designed to optimize tracking and vertexing at detector pseudorapidities of |η det | < 2.5. 1 The liquid-argon sampling calorimeter has a central section covering pseudorapidities |η det | up to ≈ 1.1, and two end calorimeters that extend coverage to |η det | ≈ 4.2, with all three housed in separate cryostats. A outer muon system, with pseudorapidity coverage of |η det | < 2, consists of a layer of tracking detectors and scintillation trigger counters in front of 1.8 T iron toroids, followed by two similar layers after the toroids.
Within the SM, the top quark decays with almost 100% probability into a W boson and a b quark. We also include two final 1 The pseudorapidity is defined as η = − ln[tan(θ/2)], where θ is the polar angle of the reconstructed particle originating from the pp collision vertex, relative to the proton beam direction. Detector pseudorapidity η det is defined relative to the center of the detector. states: the dilepton final state ( ), where both W bosons decay to leptons, and the lepton+jets final state ( +jets), where one of the W bosons decays into a pair of quarks and one decays to a lepton and a neutrino. The +jets and final states contain, respectively, one or two isolated charged leptons. In both final states we consider only electrons and muons, including those from τ -lepton decay, W → τ ν τ → ν ν τ . We also require the presence of two b quark jets, two light-quark jets from W decay (in +jets), and a significant missing transverse momentum (/ p T ) due to the escaping neutrinos.
We use the following selection criteria. In the channels, we require two isolated leptons with p T > 15 GeV, both originating from the same pp interaction vertex. The +jets channels require one isolated lepton with p T > 20 GeV. We consider electrons and muons identified using the standard D0 criteria [33,34], in the pseudorapidity range of |η det | < 2.0 for muons, and |η det | < 1.1 for electrons. In the channels, we consider in addition forward electrons in the range of 1.5 < |η det | < 2.5. Jets are reconstructed and identified from energy deposition in the calorimeter using an iterative midpoint cone algorithm [35] of radius ( φ) 2 + ( η) 2 = 0.5. Their energies are corrected using the jet energy scale (JES) algorithm [36]. All channels also require the presence of at least two jets with p T > 20 GeV and |η det | < 2.5. For the +jets final state, at least four jets must be identified with the same p T and η det cutoffs, but with the leading jet required to have p T > 40 GeV.
When a muon track is found within a jet cone, the JES calculation takes that muon momentum into account, assuming that the muon originates from the semileptonic decay of a heavy-flavor hadron belonging to the jet. To identify b quark jets, we use a multivariate b quark jet identification discriminant that combines information from the impact parameters of the tracks and variables that characterize the presence and properties of secondary vertices within the jet [37]. We require that at least one jet is identified as a b quark jet in the channels, and at least two such jets in the +jets channels. To improve signal purity, additional selections based on the global event topology are applied [38,39] in each final state. A detailed description of event selection can be found in Ref. [38] for the and in Ref. [39] for the +jets final states.
To simulate tt events we use the next-to-leading (NLO) order Monte Carlo (MC) QCD generator mc@nlo (version 3.4) [40,41], interfaced to herwig (version 6.510) [42] for parton showering and hadronization. The CTEQ6M parton distribution functions (PDF) [43,44] are used to generate events at a top quark mass of m t = 172.5 GeV. We use two samples, one including spin correlation effects, and the other without correlation. The generated events are processed through a geant3-based [45] simulation of the D0 detector. To simulate effects from additional overlapping pp interactions, "zero bias" events taken from collider data with an unbiassed trigger based solely on beam bunch crossings are overlaid on the simulated events. Simulated events are then processed with the same reconstruction program as data.
In the channels, the main sources of background are Drell-Yan production, qq → Z /γ → , diboson W W , W Z, Z Z production, and instrumental background. The instrumental background arises mainly from multijet and (W → ν)+jets events, in which one jet in W +jets or two jets in multijet events are misidentified as electrons, or where muons or electrons originating from semileptonic decay of heavy-flavor hadrons appear to be isolated. The instrumental background is determined from data, while the other backgrounds are estimated using MC simulations. For the +jets channel, in addition to the Drell-Yan and diboson production, the contribution from W +jets production is estimated from MC simulation, but normalized to data. Electroweak single top quark production and tt dilepton final states are also considered as background. The Drell-Yan and (W → ν)+jets samples Table 1 Numbers of expected events, and numbers of events found in data. are generated with the leading order (LO) matrix element generator alpgen (version v2.11) [46], interfaced to pythia [47] (version 6.409, D0 modified tune A [48]) for parton showering and hadronization. Diboson events are generated with pythia. More details about background estimation can be found in Refs. [38,39]. Table 1 shows the number of expected events for each background source and for the signal, and the number of selected events in data. The number of the expected tt events is normalized to the NLO cross section of 7.45 +0.48 −0.67 pb [49]. The observed number of events in the +jets channel is higher than the expected, mainly due to an excess in the μ+jets channel. The expected and observed number of events are consistent when the systematic uncertainties, partially correlated between the +jets and channels, are taken into account. These uncertainties are of the order of 10%. The most important contributions are the integrated luminosity, b-quark jet modeling, uncertainties on the tt modeling and uncertainty in the heavy flavor NLO K -factors of the W +jets background in the +jets channel.

Measurement technique and results
Our measurement uses the same matrix element (ME) approach as Refs. [16,50], adapted to the spin correlation measurement. This method consists of calculating the spin correlation discriminant [51] R where P tt (x, H ) is a per-event probability for hypothesis H for the vector of the reconstructed object parameters x. Hypothesis H = SM assumes the tt spin correlation strength predicted by the SM, and H = null assumes uncorrelated spins. These probabilities are calculated from the integral Here, q 1 and q 2 represent the respective fractions of proton and antiproton momentum carried by the initial state partons, f PDF represents the parton distribution functions, s is the square of the pp center-of-mass energy, and y refers to partonic final state four-  pothesis H = null, we set the spin correlation part to zero [11,12].
In the calculation, we assume perfect measurements of the lepton and jet directions, and perfect measurement of electron energy, which reduces the number of dimensions that require integration. The probability is obtained by integrating over the remaining kinematic variables. In the final state, we use the top and antitop quark masses, W + and W − boson masses, p T of two jets, 1/p T for any muons and p T and φ of the tt system as integration variables. In the +jets final state, the variables are the top and antitop quark masses, the mass of the W boson decaying to qq , p T of the d-type quark jet, p z of the leptonically decaying top quark and 1/p T of a muon. Given the inability to know the flavor of the two quarks from the W boson decay, or which b-tagged jet originates from the decay of the top or anti-top quark, all possible jet-parton assignments are considered and P tt is calculated as the sum over all the probabilities.
The distributions in the discriminant R of Eq. (1) are calculated for simulated tt events with SM spin correlation and with uncorrelated spins. These and the expected contributions from the background events are used as templates to fit the R distribution in data through a binned maximum-likelihood fit with two free parameters: the tt production cross section σ tt , and the measured fraction of events with the SM spin correlation strength, f . This fit of the distributions in the and +jets channels is performed simultaneously, with the expected number of events n i in each bin i given by where n i SM and n i null are the number of events in bin i based on the mc@nlo prediction, with and without spin correlations, and n i bckg is the expected number of background events in the same bin. We use a non-uniform bin width and require a sufficiently large number of events for each bin in order to avoid bins with zero events, as they could bias the fit result. The exact number of bins and their size were optimized to give the smallest expected statistical uncertainty in the case of the SM spin correlation. We use the same number and widths of the bins for the +jets and channels so as to keep the bin optimization procedure relatively simple. The fit yields f = 1.16 ± 0.21 (stat). The R distribution for the combined and +jets channels is shown in Fig. 1. We estimate the significance of the non-zero spin correlation hypothesis using the Feldman and Cousins frequentist procedure [52], assum- ing that the parameter f is in the range [0, 1], even though the measured value obtained in the fit is outside of the range [0, 1].
To translate the f value to the spin correlation strength in the off-diagonal basis O off , we must consider the value of the spin correlation strength in the simulation O MC off . We choose to obtain this value in the simulated samples from the expected value of k 1 k 2 O MC off = −9 cos θ 1 · cos θ 2 [14], where θ 1 and θ 2 represent angles between the respective direction of a positively and negatively charged lepton and the spin quantization axes in the t and t rest frame. The parameters k 1 and k 2 are the spin analyzingpower coefficients of the top quark (equal to 1 for leptons at LO in QCD) [53]. With mc@nlo, the value calculated for the parton-level distributions before any selections is found to equal O mc@nlo off = 0.766 in the off-diagonal basis. The measured spin correlation strength for +jets and channels is therefore We can reinterpret the measured fraction f as the related measurement of the spin correlation observable O spin = 4 3 (S t · St ) [10]. This observable characterizes the distribution in the opening angle, ϕ, between the directions of the two leptons in dilepton events or between the lepton and the up-type quark from the W decay in +jets events, where the directions are defined in the t and t rest frame:

Systematic uncertainties
The estimated systematic uncertainties are summarized in Table 2. These are obtained by replacing the nominal tt and background results with modified templates, refitting the data and determining the new fraction f .
We consider several sources of uncertainties in the modeling of the signal. These include initial-state and final-state radiation, the simulation of hadronization and underlying events, the effects of higher-order corrections, color-reconnection and uncertainty on the top quark mass. The details of the corresponding samples and parameters are discussed in Refs. [1,2].
For the PDF uncertainty, we change the 20 CTEQ6 eigenvectors independently and add the resulting uncertainties in quadrature. In modeling both the estimated signal and PDF uncertainties, the event samples have different fractional contributions from gg fusion and qq annihilation, and therefore different spin-correlation strengths. We take this into account by normalizing the measured fraction to the spin-correlation strength of the sample O MC off , in a way similar to that used for the nominal measurement off . The statistical uncertainty in MC templates is estimated using the ensemble testing technique. The new ensembles are created through a random generation of a new number of events in each bin of the MC template assuming a Gaussian distribution in the number of events in the bin. The same distribution in data is fitted with the modified templates and the dispersion in the fit results over 1000 ensembles is used as an estimation of the statistical uncertainty in the MC templates.
The uncertainty on identification and reconstruction effects includes uncertainties on lepton, jet and b tagging identification efficiencies, jet energy resolution and scale corrections, trigger efficiencies, and the luminosity. The uncertainty in the background contributions includes all uncertainties that affect the signal-tobackground ratio that are not contained in the previous categories. These uncertainties include uncertainties in theoretical cross sections for backgrounds, uncertainty in Z boson p T distribution, and uncertainties in instrumental background contributions.
The total absolute systematic uncertainty on the spin correlation observable O meas off , calculated as a quadratic sum over all individual sources, is 0.15, as shown in Table 2.

Spin correlation and the tt production mechanism
The strength of the tt spin correlation in the SM is strongly dependent on the tt production mechanism. The spin correlation measurement thus provides a way of measuring the fraction of events produced via gg fusion, f gg [13]. The f gg fraction is not well defined at orders higher than LO QCD. The difficulty arises from the fact that the cross sections for the gq → ttq and gq → ttq processes at LO, as well as gg and qq production at NLO, contain a singularity when the final state quark is collinear with the quark in the initial state. This makes the integration over the phase space divergent [15,54,55]. In practice, this singularity is absorbed into the definition of the PDF, but the final results depend on the scheme used for regularization. For the NLO PDF, the MS scheme is usually preferred. The gq and gq contribution at NLO is of the order of a few percent [10,14,15], and considering that the overall spin correlation strength is ≈ 80%, we neglect these smaller contributions, and determine f gg from the relation Assuming O qq ≈ 1, the gluon fraction becomes where O is the measured value of the total spin correlation strength, and O gg is the SM value of the spin correlation strength for gg events. The NLO calculation in the off-diagonal basis using the CT10 PDF yields O gg = −0.36 ± 0.02 [10,14,15]. The systematic uncertainty on the observable O can be translated to the uncertainty on the gluon fraction that includes an additional contribution from the theoretical uncertainty on O gg . In the absence of non-SM contributions, the fraction of tt events produced through gluon fusion becomes f gg = 0.08 ± 0.12(stat) ± 0.11(syst) = 0.08 ± 0.16(stat + syst) , in agreement with the NLO prediction of f gg = 0.135 [10,14,15].

Summary
We have presented an updated measurement of tt spin correlations with the D0 detector for an integrated luminosity of 9.7 fb −1 . The result of the measurement of the strength of the tt spin correlation in the off-diagonal basis is O off = 0.89 ± 0.16 (stat) ± 0.15 (syst) = 0.89 ± 0.22 (stat + syst). This result is in agreement with the NLO QCD calculation O off = 0.80 +0.01 −0.02 [10] and supersedes that reported in Ref. [16]. Using the Feldman and Cousins approach for interval setting [52], and assuming uncorrelated tt spins, we estimate a probability (p-value) of 2.5 × 10 −5 for obtaining a spin correlation larger than the observed value. This corresponds to evidence for spin correlation in tt events at a significance of 4.2 standard deviations.
In the absence of non-SM contributions, we use the spin correlation strength measurement to constrain the fraction of events produced through gluon fusion at NLO QCD and obtain f gg = 0.08 ± 0.16(stat + syst) , in good agreement with SM prediction.