# A precise determination of the top-quark pole mass

- 200 Downloads
- 2 Citations

## Abstract

The Principle of Maximum Conformality (PMC) provides a systematic way to eliminate the renormalization scheme and renormalization scale uncertainties for high-energy processes. We have observed that by applying PMC scale setting, one obtains comprehensive and self-consistent pQCD predictions for the top-quark pair total cross section and the top-quark pair forward–backward asymmetry in agreement with the measurements at the Tevatron and LHC. As a step forward, in the present paper, we determine the top-quark pole mass via a detailed comparison of the top-quark pair cross section with the measurements at the Tevatron and LHC. The results for the top-quark pole mass are \(m_t=174.6^{+3.1}_{-3.2}\) GeV for the Tevatron with \(\sqrt{S}=1.96\) TeV, \(m_t=173.7\pm 1.5\) and \(174.2\pm 1.7\) GeV for the LHC with \(\sqrt{S} = 7\) and 8 TeV, respectively. Those predictions agree with the average, \(173.34\pm 0.76\) GeV, obtained from various collaborations via direct measurements. The consistency of the pQCD predictions using the PMC with all of the collider measurements at different energies provides an important verification of QCD.

## 1 Introduction

The top quark is the heaviest particle of the Standard Model (SM), and its mass is one of the fundamental parameters within the SM. The large top-quark mass implies a strong top-quark Yukawa coupling to the Higgs boson, playing a special role in testing the electroweak symmetry breaking mechanism and for the search of new physics beyond the SM. The top quark decays before hadronization, and one can determine its mass by directly measuring its decay products [1]. Such measurements allow for the direct extraction of the top-quark mass (\(m_t\)), which however, relies heavily on the detailed reconstruction of the kinematics and reconstruction efficiency [2, 3]. In 2014, a combination of measurements of the top-quark mass performed by the CDF and D0 experiments at the Tevatron collider and the ATLAS and CMS experiments at the Large Hadron Collider (LHC) gives [4], \(m_t\,{=}\,173.34\,{\pm }\,0.76\) GeV. The direct measurements are based on analysis techniques which use top-pair events provided by Monte Carlo (MC) simulation for different assumed values of the top-quark mass. Applying those techniques to data yields a mass quantity corresponding to the top-quark mass scheme implemented in the MC, thus it is referred as the “MC mass”.

Another important approach for extracting the top-quark mass is done by using detailed comparisons of the pQCD predictions with the corresponding measurements; this method is indirect, but it provides complementary information on the top quark compared to direct measurements. Theoretical arguments suggest that the top-quark MC mass is within \(\sim 1\) GeV of its pole mass [5], and thus its use has a negligible effect on the determination of pole mass [6, 7].^{1} Thus in our present calculations, we shall only extract the top-quark pole mass and as usual directly take the determined top-quark MC mass by the experimental groups as the value of the top-quark pole mass. Recently, such indirect extractions of \(m_t\) from the top-quark pair production channels by various experimental collaborations have been performed, giving the pole value, \(m_t=173.8^{+1.7}_{-1.8}\) GeV from CMS [7], \(m_t=172.8^{+3.4}_{-3.2}\) GeV from D0 [10], and \(m_t=172.9^{+2.5}_{-2.6}\) GeV from ATLAS [11].

A key goal for the indirect determinations is to have a precise theoretical prediction for the top-quark pair production cross section in order to provide maximal constraints on \(m_t\). Practically, one can first set an arbitrary initial renormalization scale to do the pQCD calculation, whose value only need to be large enough to ensure the applicability of the pQCD theory. Under conventional scale setting, the renormalization scale is fixed to its initial value, which is usually chosen as the typical momentum flow of the process or the one to eliminate large logs in the perturbative series. More explicitly, it is conventional to take the renormalization scale in those predictions as the top-quark mass \(m_{t}\) to eliminate the large logarithmic terms such as \(\ln (\mu _r/m_{t})\); one then varies the renormalization scale over an arbitrary range such as \([m_{t}/2, 2m_{t}]\) to ascertain the uncertainty. At sufficiently high order, a small renormalization scale-dependent prediction may be achieved for global quantities such as the total cross section. However, such small renormalization scale dependence of the resulting prediction is due to cancelations among different orders; the renormalization scale uncertainty for each order is still uncertain and could be very large. In fact, when one applies conventional scale setting, the renormalization scheme- and initial renormalization scale-dependence is introduced at any fixed order.

The Principle of Maximum Conformality (PMC) [12, 13, 14, 15, 16] provides a systematic way to eliminate renormalization scheme-and-scale ambiguities. It generalizes the BLM scale-setting procedure [17] to all orders. As in QED [18], one shifts the argument of the running coupling at each order in the pQCD series to absorb all occurrences of the \(\beta \)-function. In addition, a convergent pQCD series without factorial renormalon divergence can be obtained. The PMC predictions are renormalization-scheme independent at each order in \(\alpha _s\), since all of the scheme-dependent \(\{\beta _i\}\)-terms in the QCD perturbative series have been resummed into the running couplings. The PMC satisfies renormalization group invariance and satisfies all of the self-consistency conditions of the renormalization group [19, 20], and it reduces in the \(N_C\rightarrow 0\) Abelian limit [21] to the standard Gell-Mann-Low method [18]. A number of PMC applications are summarized in the review [22]; in each case the PMC works successfully and leads to improved agreement with experiment.

By applying PMC scale setting, we can achieve optimal renormalization scales of the process and thus obtain precise predictions for the top-quark pair production cross section without conventional renormalization scale uncertainty [23, 24, 25, 26]. Because of the uncalculated high-order terms, there is residual renormalization scale dependence for the PMC prediction. However, such residual renormalization scale dependence is generally small either due to the perturbative nature of the PMC scales or due to the fast convergence of the conformal pQCD series; e.g. we have found that the residual renormalization for top-pair production is negligibly small at the NNLO level. The PMC predictions for the top-quark pair forward–backward asymmetry are also in agreement with the corresponding CDF and D0 measurements [27], since it correctly assigns different renormalization scales in the one- and two-gluon exchange amplitudes.

In subsequent sections, we will determine the top-quark pole mass from a detailed comparison of the top-quark pair production cross section predicted by applying the PMC with the measured values obtained by the Tevatron and LHC experiments.

## 2 Top-quark pair production at the hadron colliders and the determination of top-quark pole mass

*S*denotes the hadronic center-of-mass energy squared, and \(s=x_1 x_2 S\) is the subprocess center-of-mass energy squared. The parameter \(\mu _r\) denotes the (initial) renormalization scale and \(\mu _f\) denotes the factorization scale. The choice of \(\mu _r\) is arbitrary, which is only need to be in pQCD region (\(\gg \Lambda _\mathrm{QCD}\)) and usually people set its value as the typical momentum flow of the process; and for this process, \(\mu _r\) is usually chosen as \(m_t\). The function \(f_{i/H_{\alpha }}(x_\alpha ,\mu _f)\) (\(\alpha =1\) or 2) describes the probability of finding a parton of type

*i*with a light-front momentum fraction between \(x_\alpha \) and \(x_{\alpha } +dx_{\alpha }\) in the proton \(H_{\alpha }\).

In doing the numerical analysis, we will first take the top-quark pole mass as \(m_t=173.3\) GeV [41] and choose the parton distribution functions (PDF) as the CT14 version of the CTEQ collaboration [42]. The NNLO \(\alpha _s\)-running is adopted with its normalization fixed in \(\overline{\mathrm{MS}}\)-scheme using \(\alpha _s(M_Z)=0.118\).

^{2}; however, a possible determination can be based on the light-front holographic QCD [44]. It determines a scale \(Q_0\) at the interface between nonpertubative and perturbative QCD. In the analysis given here, we will take \(\mu _f=m_t\).

The NNLO top-quark pair production cross sections for the Tevatron and LHC (in unit: pb), comparing conventional versus PMC scale settings. Here all production channels have been summed up. Three typical choices for the initial renormalization scales \(\mu _{r}=m_t/2\), \(m_t\) and \(2m_t\) have been adopted

Conventional | PMC | |||||
---|---|---|---|---|---|---|

\(\mu _r\) | \(m_t/2\) | \(m_t\) | \(2m_t\) | \(m_t/2\) | \(m_t\) | \(2m_t\) |

\(\sigma ^{1.96\mathrm TeV}_\mathrm{Tevatron}\) | 7.54 | 7.29 | 7.01 | 7.43 | 7.43 | 7.43 |

\(\sigma ^{7\mathrm TeV}_\mathrm{LHC}\) | 172.07 | 167.67 | 160.46 | 174.97 | 174.98 | 174.99 |

\(\sigma ^{8\mathrm TeV}_\mathrm{LHC}\) | 244.87 | 239.03 | 228.94 | 249.16 | 249.18 | 249.19 |

\(\sigma ^{13\mathrm TeV}_\mathrm{LHC}\) | 792.36 | 777.72 | 746.92 | 807.80 | 807.83 | 807.86 |

We present the NNLO top-quark pair production cross section at the hadronic colliders Tevatron and LHC for both conventional and PMC scale settings in Table 1, where three typical initial renormalization scales are adopted. The results shown in Table 1 show that if one uses conventional scale setting, the renormalization scale dependence of the NNLO cross section is still about 6–7% for \(\mu _r\in [m_t/2, 2m_t]\). If one analyzes the pQCD series in detail, one finds that the dependence of the NNLO cross section on the guess of the renormalization scale using conventional scale setting is due to cancelations among different orders, and the renormalization scale dependence of each perturbative term is rather large [27]. Thus computing a finite number of additional higher-order terms could soften the renormalization scale dependence for the total cross section to a certain degree, but it does not eliminate the dependence on the choice of the initial renormalization scale, especially when the detailed dependence on the renormalization scales at each order is also important.

When PMC scale setting is used, the renormalization scales are fixed by using the renormalization group equation recursively, thus fixing the arguments of the strong couplings at each order. There is residual renormalization scale dependence due to unknown NNNLO and higher-order contributions, for example, we need to known the \(\beta \)-terms at the NNNLO level to fix the PMC scale of the NNLO-terms. Table 1 shows that the residual renormalization scale dependence of the NNLO total cross section is negligibly small for \(\mu _r\in [m_t/2, 2 m_t]\), which is less than \(0.1\%\) even when taking a quite large initial renormalization scale range \(\mu _r\in [m_t/4, 20m_t]\). The PMC scales are distinct at different orders, as in QED. Since the PMC scales are determined from perturbative input, any renormalization scale uncertainty of the pQCD series is transferred at finite order to the small uncertainty of the PMC scales.

If setting \(\mu _r=m_t/2\) for conventional scale setting, the pQCD convergence is better than the cases of \(\mu _r=m_t\) and \(\mu _r=2m_t\), whose total cross section is also close to the PMC prediction. Thus, for conventional scale setting, the best choice of an effective renormalization scale for top-quark pair production is \(\mu _r\sim m_t/2\) other than the conventional suggested \(m_t\) [26]. The choice of \(\mu _r\sim m_t/2\) is also suggested in Ref. [45] by using the principle of fastest perturbative convergence.

The coefficients \(c_{0,1,2,3}\) as determined from the PMC predictions for the top-quark pair cross section by varying the top-quark pole mass from 160 GeV to 190 GeV. The notation \([\sigma _\mathrm{th}(m_t) + \Delta \sigma ^{+}_\mathrm{th}(m_t)]\) indicates that the coefficients are determined using the maximum cross section within its allowable parameter range, and \([\sigma _\mathrm{th}(m_t)-\Delta \sigma ^{-}_\mathrm{th}(m_t)]\) corresponds to the minimum cross section

\(c_0 [\mathrm pb]\) | \(c_1 [\mathrm pb]\) | \(c_2 [\mathrm pb]\) | \(c_3 [\mathrm pb]\) | |
---|---|---|---|---|

Tevatron | ||||

\(\sigma _\mathrm{th}\) | 7.6181 | \(-\) 0.06140 | \(2.1135\times 10^{-4}\) | \(-\,1.9319\times 10^{-6}\) |

\(\sigma _\mathrm{th}+\Delta \sigma ^{+}_\mathrm{th}\) | 7.7580 | \(-\) 0.06261 | \(2.1711\times 10^{-4}\) | \(-\,1.9923\times 10^{-6}\) |

\(\sigma _\mathrm{th}-\Delta \sigma ^{-}_\mathrm{th}\) | 7.4796 | \(-\) 0.06019 | \(2.0572\times 10^{-4}\) | \(-\,1.8750\times 10^{-6}\) |

LHC\(|_{7\mathrm TeV}\) | ||||

\(\sigma _\mathrm{th}\) | 179.2422 | \(-\) 1.2311 | \( 4.7155\times 10^{-3}\) | \(-\,3.3920\times 10^{-5}\) |

\(\sigma _\mathrm{th}+\Delta \sigma ^{+}_\mathrm{th}\) | 182.8195 | \(-\) 1.2590 | \( 4.8479\times 10^{-3}\) | \(-\,3.5338\times 10^{-5}\) |

\(\sigma _\mathrm{th}-\Delta \sigma ^{-}_\mathrm{th}\) | 175.7093 | \(-\) 1.2037 | \( 4.5866\times 10^{-3}\) | \(-\,3.2489\times 10^{-5}\) |

LHC\(|_{8\mathrm TeV}\) | ||||

\(\sigma _\mathrm{th}\) | 255.0975 | \(-\) 1.5718 | \( 5.2644\times 10^{-3}\) | \(-\,4.2394\times 10^{-5}\) |

\(\sigma _\mathrm{th}+\Delta \sigma ^{+}_\mathrm{th}\) | 260.1779 | \(-\) 1.6078 | \( 5.4191\times 10^{-3}\) | \(-\,4.4240\times 10^{-5}\) |

\(\sigma _\mathrm{th}-\Delta \sigma ^{-}_\mathrm{th}\) | 250.0801 | \(-\) 1.5364 | \( 5.1128\times 10^{-3}\) | \(-\,4.0618\times 10^{-5}\) |

LHC\(|_{13\mathrm TeV}\) | ||||

\(\sigma _\mathrm{th}\) | 825.5955 | \(-\) 3.2873 | \(5.1997\times 10^{-3}\) | \(-\,1.0274\times 10^{-4}\) |

\(\sigma _\mathrm{th}+\Delta \sigma ^{+}_\mathrm{th}\) | 841.9260 | \(-\) 3.3675 | \(5.4202\times 10^{-3}\) | \(-\,1.0730\times 10^{-4}\) |

\(\sigma _\mathrm{th}-\Delta \sigma ^{-}_\mathrm{th}\) | 809.4638 | \(-\) 3.2084 | \(4.9863\times 10^{-3}\) | \(-\,9.8738\times 10^{-5}\) |

It is important to study the ratio of total cross sections \(R^{8/7}=(\sigma ^{8\mathrm TeV}_\mathrm{LHC})/(\sigma ^{7\mathrm TeV}_\mathrm{LHC})\), since the experimental uncertainties, which are correlated between the two analyses (at \(\sqrt{S}\) = 7 or 8 TeV) cancel out, leading to an improved precision in comparison to the individual measurements. The predicted cross-section ratio by the PMC is \(R^{8/7}|_\mathrm{PMC}=1.42\pm 0.04\), which shows excellent agreement with the latest CMS measurement \(R^{8/7}|_\mathrm{CMS}= 1.43\pm 0.04 \pm 0.07 \pm 0.05\) [53].

As we have shown above, the PMC provides a comprehensive and self-consistent pQCD explanation for the top-quark pair production cross section as well as the top-quark pair forward–backward asymmetry. The behavior of the top-quark pair production cross section allows a direct determination of the top-quark pole mass by comparing the pQCD prediction with the data.

We present the top-quark pair NNLO production cross section (5) versus the top-quark pole mass at different hadron-hadron collision energies in Figs. 2 and 3. The coefficients \(c_{0,1,2,3}\) are determined by the PMC predictions. In these figures, the experimental measurements are presented for comparison, where the thinnest shaded bands are for the PMC predictions and the thickest shaded bands are for the combined experimental results, respectively. The agreement of the PMC predictions with the measurements, as shown by Figs. 2 and 3, makes it possible to achieve reliable predictions for top-quark pole mass. A precise range of values for the pole mass can thus be achieved in comparison with pQCD predictions based on conventional scale setting. In the following, we will determine the top-quark pole mass such that the maximum value of the likelihood function (3) is achieved.

Top-quark pole mass (in unit GeV) determined by CMS and ATLAS collaborations at \(\sqrt{S}=7\) TeV [2, 7, 11, 64], where the theoretical predictions for top-quark pair production is based on conventional (Conv.) scale setting. Our predictions using PMC scale setting are presented as a comparison

By using the measured cross section \(\sigma _\mathrm{exp}(m_t)\) together with its error \(\Delta \sigma _\mathrm{exp}(m_t)\) from the latest CMS measurement [7], we present the likelihood functions at the LHC in Fig. 5. Because the experimental uncertainty at the LHC is smaller than that of Tevatron, the determined top-quark pole mass by using the LHC data has better precision in comparison with the analysis using the Tevatron data. By evaluating the likelihood functions, we obtain \(m_t=173.7\pm 1.5\) GeV for \(\sqrt{S}=7\) TeV, and \(m_t=174.2\pm 1.7\) GeV for \(\sqrt{S}=8\) TeV. The precision of the top-quark pole masses determination is improved to be (\({\pm 1.5}\)) for \(\sqrt{S}=7\) TeV and (\({\pm 1.7}\)) for \(\sqrt{S}=8\) TeV.

We summarize the top-quark pole masses determined at both Tevatron and LHC in Fig. 6, where our PMC predictions and previous predictions from other collaborations [2, 3, 7, 10, 11, 68, 71, 72] are presented. For reference, the combination of Tevatron and LHC direct measurements of the top-quark mass is presented as a shaded band, giving \(m_t=173.34\pm 0.76\) GeV [4]. It shows that our new top-quark pole mass determined by PMC agree with the combination of Tevatron and LHC direct measurements.

## 3 Summary

We have achieved precise predictions for the top-quark pair production cross section with minimal dependence on the choice of the initial renormalization scale by using PMC. The resulting predictions are in agreement with measurements done by both the Tevatron and the LHC collaborations. We have given a new determination of the top-quark pole mass by comparing the PMC prediction for the top-quark pair cross sections with the latest measurements; a detailed comparison of previous determinations given in the literature has also been presented. Our new determination of the top-quark pole masses provide complementary information compared to direct measurements.

The determined top-quark pole masses are cross-checked by other determinations used different techniques. Typically, the mass \(m_t=175.8^{+2.7}_{-2.4}\) GeV from an electroweak fits [73], the mass \(m_t=173.5\pm 3.0\pm 0.9\) GeV reconstructed from lepton + \(J/\psi \) from b-jet [74], the mass \(m_t=173.2\pm 1.6\) GeV from dilepton kinematic distributions [75] and the best direct measurement results \(m_t=172.99\pm 0.85\) GeV from ATLAS [76] and \(m_t=172.35\pm 0.51\) GeV from CMS [77]. The consistency of the pQCD predictions using the PMC with all of the collider measurements at different energies and different techniques provides an important verification of QCD.

The PMC provides a systematic, rigorous method for eliminating renormalization scheme-and-scale ambiguities at each order in perturbation theory. As we have shown in our previous papers, the PMC is applicable to a wide variety of perturbatively calculable processes. In each case, the ad hoc renormalization scale uncertainty conventionally assigned to the pQCD predictions can be eliminated. The residual renormalization scale dependence due to uncalculated high-order terms are usually small due to a more convergent pQCD series. The PMC, with its solid physical and rigorous theoretical background, thus will greatly improve the precision of tests of the Standard Model.

## Footnotes

## Notes

### Acknowledgements

The authors would like to thank Hui-Lan Liu for helpful discussions. This work was supported in part by the Natural Science Foundation of China under Grant No. 11547010, No. 11625520, No. 11705033 and No. 11325525; by the Project of Guizhou Provincial Department of Science and Technology under Grant No. 2016GZ42963 and the Key Project for Innovation Research Groups of Guizhou Provincial Department of Education under Grant No. KY[2016]028 and No. KY[2017]067; and by the Department of Energy Contract No. DE-AC02-76SF00515. SLAC-PUB-16934.

## References

- 1.R.H. Dalitz, G.R. Goldstein, Phys. Lett. B
**287**, 225 (1992)ADSCrossRefGoogle Scholar - 2.S. Chatrchyan et al. [CMS Collaboration], Phys. Lett. B
**728**, 496 (2014) (Erratum: [Phys. Lett. B**738**, 526 (2014)])Google Scholar - 3.M. Aaboud et al. [ATLAS Collaboration], ATLAS-CONF-2011-054Google Scholar
- 4.[ATLAS and CDF and CMS and D0 Collaborations], arXiv:1403.4427 [hep-ex]
- 5.A. Buckley et al., Phys. Rep.
**504**, 145 (2011)ADSCrossRefGoogle Scholar - 6.S. Fleming, A.H. Hoang, S. Mantry, I.W. Stewart, Phys. Rev. D
**77**, 074010 (2008)ADSCrossRefGoogle Scholar - 7.V. Khachatryan et al., [CMS Collaboration]. JHEP
**1608**, 029 (2016)Google Scholar - 8.R. Tarrach, Nucl. Phys. B
**183**, 384 (1981)ADSCrossRefGoogle Scholar - 9.A.S. Kronfeld, Phys. Rev. D
**58**, 051501 (1998)ADSCrossRefGoogle Scholar - 10.V.M. Abazov et al., [D0 Collaboration]. Phys. Rev. D
**94**, 092004 (2016)Google Scholar - 11.G. Aad et al., [ATLAS Collaboration]. Eur. Phys. J. C
**74**, 3109 (2014)Google Scholar - 12.X.G. Wu, S.J. Brodsky, M. Mojaza, Prog. Part. Nucl. Phys.
**72**, 44 (2013)ADSCrossRefGoogle Scholar - 13.S.J. Brodsky, X.G. Wu, Phys. Rev. D
**85**, 034038 (2012) [Phys. Rev. D**86**, 079903 (2012)]Google Scholar - 14.S.J. Brodsky, L. Di Giustino, Phys. Rev. D
**86**, 085026 (2012)ADSCrossRefGoogle Scholar - 15.M. Mojaza, S.J. Brodsky, X.G. Wu, Phys. Rev. Lett.
**110**, 192001 (2013)ADSCrossRefGoogle Scholar - 16.S.J. Brodsky, M. Mojaza, X.G. Wu, Phys. Rev. D
**89**, 014027 (2014)ADSCrossRefGoogle Scholar - 17.S.J. Brodsky, G.P. Lepage, P.B. Mackenzie, Phys. Rev. D
**28**, 228 (1983)ADSCrossRefGoogle Scholar - 18.M. Gell-Mann, F.E. Low, Phys. Rev.
**95**, 1300 (1954)ADSCrossRefGoogle Scholar - 19.S.J. Brodsky, X.G. Wu, Phys. Rev. D
**86**, 054018 (2012)ADSCrossRefGoogle Scholar - 20.X.G. Wu, Y. Ma, S.Q. Wang, H.B. Fu, H.H. Ma, S.J. Brodsky, M. Mojaza, Rep. Prog. Phys.
**78**, 126201 (2015)ADSCrossRefGoogle Scholar - 21.S.J. Brodsky, P. Huet, Phys. Lett. B
**417**, 145 (1998)ADSMathSciNetCrossRefGoogle Scholar - 22.X.G. Wu, S.Q. Wang, S.J. Brodsky, Front. Phys.
**11**, 111201 (2016)CrossRefGoogle Scholar - 23.S.J. Brodsky, X.G. Wu, Phys. Rev. Lett.
**109**, 042002 (2012)ADSCrossRefGoogle Scholar - 24.S.J. Brodsky, X.G. Wu, Phys. Rev. D
**86**, 014021 (2012)ADSCrossRefGoogle Scholar - 25.S.J. Brodsky, X.G. Wu, Phys. Rev. D
**85**, 114040 (2012)ADSCrossRefGoogle Scholar - 26.S.Q. Wang, X.G. Wu, Z.G. Si, S.J. Brodsky, Phys. Rev. D
**90**, 114034 (2014)ADSCrossRefGoogle Scholar - 27.S.Q. Wang, X.G. Wu, Z.G. Si, S.J. Brodsky, Phys. Rev. D
**93**, 014004 (2016)ADSCrossRefGoogle Scholar - 28.P. Nason, S. Dawson, R.K. Ellis, Nucl. Phys. B
**303**, 607 (1988)ADSCrossRefGoogle Scholar - 29.P. Nason, S. Dawson, R.K. Ellis, Nucl. Phys. B
**327**, 49 (1989)ADSCrossRefGoogle Scholar - 30.W. Beenakker, H. Kuijf, W.L. van Neerven, J. Smith, Phys. Rev. D
**40**, 54 (1989)ADSCrossRefGoogle Scholar - 31.W. Beenakker, W.L. van Neerven, R. Meng, G.A. Schuler, J. Smith, Nucl. Phys. B
**351**, 507 (1991)ADSCrossRefGoogle Scholar - 32.M. Czakon, A. Mitov, Nucl. Phys. B
**824**, 111 (2010)ADSCrossRefGoogle Scholar - 33.S. Moch, P. Uwer, Phys. Rev. D
**78**, 034003 (2008)ADSCrossRefGoogle Scholar - 34.M. Beneke, P. Falgari, S. Klein, C. Schwinn, Nucl. Phys. B
**855**, 695 (2012)ADSCrossRefGoogle Scholar - 35.N. Kidonakis, Phys. Rev. D
**82**, 114030 (2010)ADSCrossRefGoogle Scholar - 36.P. Bärnreuther, M. Czakon, A. Mitov, Phys. Rev. Lett.
**109**, 132001 (2012)ADSCrossRefGoogle Scholar - 37.M. Czakon, A. Mitov, JHEP
**1301**, 080 (2013)ADSCrossRefGoogle Scholar - 38.M. Czakon, P. Fiedler, A. Mitov, Phys. Rev. Lett.
**110**, 252004 (2013)ADSCrossRefGoogle Scholar - 39.M. Aliev, H. Lacker, U. Langenfeld, S. Moch, P. Uwer, M. Wiedermann, Comput. Phys. Commun.
**182**, 1034 (2011)ADSCrossRefGoogle Scholar - 40.M. Czakon, A. Mitov, Comput. Phys. Commun.
**185**, 2930 (2014)ADSCrossRefGoogle Scholar - 41.The ATLAS and CMS Collaborations, ATLAS-CONF-2012-095, CMS-PAS-TOP-12-001Google Scholar
- 42.S. Dulat et al., Phys. Rev. D
**93**, 033006 (2016)ADSCrossRefGoogle Scholar - 43.S.Q. Wang, X.G. Wu, S.J. Brodsky, M. Mojaza, Phys. Rev. D
**94**, 053003 (2016)ADSCrossRefGoogle Scholar - 44.S.J. Brodsky, G.F. de Teramond, H.G. Dosch, J. Erlich, Phys. Rep.
**584**, 1 (2015)ADSMathSciNetCrossRefGoogle Scholar - 45.M. Czakon, D. Heymes, A. Mitov, JHEP
**1704**, 071 (2017)ADSCrossRefGoogle Scholar - 46.T.A. Aaltonen et al., [CDF and D0 Collaborations]. Phys. Rev. D
**89**, 072001 (2014)Google Scholar - 47.S. Chatrchyan et al., [CMS Collaboration]. JHEP
**1305**, 065 (2013)Google Scholar - 48.G. Aad et al., [ATLAS Collaboration]. Eur. Phys. J. C
**73**, 2328 (2013)Google Scholar - 49.S. Chatrchyan et al., [CMS Collaboration]. Eur. Phys. J. C
**73**, 2386 (2013)Google Scholar - 50.G. Aad et al., [ATLAS Collaboration]. Phys. Rev. D
**92**, 072005 (2015)Google Scholar - 51.S. Chatrchyan et al., [CMS Collaboration]. Phys. Rev. D
**85**, 112007 (2012)Google Scholar - 52.G. Aad et al., [ATLAS Collaboration]. Phys. Lett. B
**711**, 244 (2012)Google Scholar - 53.S. Chatrchyan et al., [CMS Collaboration]. Eur. Phys. J. C
**77**, 15 (2017)Google Scholar - 54.V. Khachatryan et al., [CMS Collaboration]. Eur. Phys. J. C
**76**, 128 (2016)Google Scholar - 55.V. Khachatryan et al., [CMS Collaboration]. Phys. Lett. B
**739**, 23 (2014)Google Scholar - 56.G. Aad et al., [ATLAS Collaboration]. Phys. Rev. D
**91**, 112013 (2015)Google Scholar - 57.V. Khachatryan et al. [CMS Collaboration], arXiv:1611.04040 [hep-ex]
- 58.V. Khachatryan et al., [CMS Collaboration]. Phys. Rev. Lett.
**116**, 052002 (2016)Google Scholar - 59.M. Aaboud et al. [ATLAS Collaboration], ATLAS-CONF-2015-049Google Scholar
- 60.M. Aaboud et al., [ATLAS Collaboration]. Phys. Lett. B
**761**, 136 (2016)Google Scholar - 61.V.M. Abazov et al., [D0 Collaboration]. Phys. Lett. B
**679**, 177 (2009)Google Scholar - 62.V.M. Abazov et al., [D0 Collaboration]. Phys. Lett. B
**704**, 403 (2011)Google Scholar - 63.V.M. Abazov et al., [D0 Collaboration]. Phys. Rev. D
**84**, 012008 (2011)Google Scholar - 64.S. Chatrchyan et al., [CMS Collaboration]. JHEP
**1211**, 067 (2012)Google Scholar - 65.S. Chatrchyan et al., [CMS Collaboration]. Phys. Lett. B
**720**, 83 (2013)Google Scholar - 66.S. Chatrchyan et al. [CMS Collaboration], JHEP
**1402**, 024 (2014) Erratum: [JHEP**1402**, 102 (2014)]Google Scholar - 67.M. Beneke, P. Falgari, S. Klein, J. Piclum, C. Schwinn, M. Ubiali, F. Yan, JHEP
**1207**, 194 (2012)ADSCrossRefGoogle Scholar - 68.V.M. Abazov et al., [D0 Collaboration]. Phys. Lett. B
**703**, 422 (2011)Google Scholar - 69.P. Marquard, A.V. Smirnov, V.A. Smirnov, M. Steinhauser, Phys. Rev. Lett.
**114**, 142002 (2015)ADSCrossRefGoogle Scholar - 70.A.L. Kataev, V.S. Molokoedov, Eur. Phys. J. Plus
**131**, 271 (2016)CrossRefGoogle Scholar - 71.V.M. Abazov et al., [D0 Collaboration]. Phys. Rev. D
**80**, 071102 (2009)Google Scholar - 72.G. Aad et al., [ATLAS Collaboration]. JHEP
**1510**, 121 (2015)Google Scholar - 73.M. Baak et al., Eur. Phys. J. C
**72**, 2205 (2012)ADSCrossRefGoogle Scholar - 74.V. Khachatryan et al., [CMS Collaboration]. JHEP
**1612**, 123 (2016)Google Scholar - 75.G. Aad et al. [ATLAS Collaboration], ATLAS-CONF-2017-044Google Scholar
- 76.M. Aaboud et al., [ATLAS Collaboration]. Phys. Lett. B
**761**, 350 (2016)Google Scholar - 77.V. Khachatryan et al., [CMS Collaboration]. Phys. Rev. D
**93**, 072004 (2016)Google Scholar

## Copyright information

**Open Access**This article is distributed under the terms of the Creative Commons Attribution 4.0 International License (http://creativecommons.org/licenses/by/4.0/), which permits unrestricted use, distribution, and reproduction in any medium, provided you give appropriate credit to the original author(s) and the source, provide a link to the Creative Commons license, and indicate if changes were made.

Funded by SCOAP^{3}