DESY 08-027

TTP08-14

SFB/CPP-08-21

April 2008

Theoretical status and prospects

[1ex] for top-quark pair production at hadron colliders

S. Moch and P. Uwer

Deutsches Elektronensynchrotron DESY

Platanenallee 6, D–15738 Zeuthen, Germany

Institut für Theoretische Teilchenphysik, Universität Karlsruhe

D–76128 Karlsruhe, Germany

Abstract

We present an update of the theoretical predictions for the cross section of top-quark pair production at Tevatron and LHC. In particular we employ improvements due to soft gluon resummation at next-to-next-to-leading logarithmic accuracy. We expand the resummed results and derive analytical finite-order cross sections through next-to-next-to-leading order which are exact in all logarithmically enhanced terms near threshold. These results are the best present estimates for the top-quark pair production cross section. We investigate the scale dependence as well as the sensitivity on the parton luminosities.

## 1 Introduction

Top-quark pair production at the LHC is important as the collider will accumulate very high statistics for this process. In the initial low luminosity run () approximately top-quark pairs will be produced per year [1, 2]. This data will allow for numerous measurements, e.g. of the top-quark mass, the electric charge of the top-quark or the weak couplings. Furthermore the data will allow precise tests of the production and the subsequent decay mechanism including anomalous couplings and top-quark spin correlations. See for example Ref. [3] for a recent review on top-quark physics at hadron colliders.

A necessary prerequisite which all these studies share in common is, of course, a detailed understanding of the production process. In Quantum Chromodynamics (QCD) this includes the radiative corrections to the cross section of heavy-quark hadro-production at the next-to-leading order (NLO) [4, 5, 6] together with its scale dependence as well as the dependence on the parton luminosities through the parton distribution functions (PDFs) of the proton. Further improvements of the perturbative stability through resummation of large Sudakov logarithms to next-to-leading logarithmic (NLL) accuracy have been considered as well [7, 8] and employed to generate approximate results at the next-to-next-to-leading order (NNLO) in QCD [9]. Very recently also an estimate of bound state effects has been presented [10].

In particular our knowledge on the parton luminosities has constantly improved over the last years. Thus, it is an imminent question how these improvements in the determination of the parton distribution functions from global fits affect predictions for physical cross sections at LHC, which are sensitive to the gluon distribution function in the regime where . For LHC observables this aspect has been quantitatively approached very recently by investigating correlations of rates for top-quark pair production with other cross sections [11]. For Tevatron, which to date has provided us with a lot of information on the top-quark, most prominently a very precise determination [12] of its mass, GeV, the cross section in Eq. (1) had been studied some time ago [13, 14]. However, due to changes in the available PDF sets from global fits an update also seems to be in order here as well.

It is the aim of this article to review theoretical predictions for the production cross sections of top-quark pairs at Tevatron and LHC and to establish the present theoretical uncertainty. We provide an update of the NLL resummed cross section as defined in Ref. [8] (and also used in Ref. [14]). Subsequently, we extend these results to the next-to-next-to-leading logarithmic (NNLL) accuracy and derive approximate NNLO cross sections thereby improving previous calculations [9, 13]. At two loops we are thus in a position to present all logarithmically enhanced terms near threshold and to assess their phenomenological impact by studying the quality of the perturbative expansion, i.e. the properties of apparent convergence and the stability under scale variations. This seems particularly interesting considering not only the anticipated experimental precision at LHC [1, 2] but also in view of recent activities aiming at complete NNLO QCD predictions for heavy-quark hadro-production [15, 16, 17, 18, 19].

The paper is organized as follows. In Sec. 2 we set the stage and study the threshold sensitivity of the inclusive hadronic cross section for top-quark pair production. Subsequently, we provide updates of Refs. [8, 14] employing recent sets of PDFs. In Sec. 3 we extend the resummed cross section to NNLL accuracy and calculate the complete logarithmic dependence of the cross section near threshold (including the Coulomb corrections). Together with the exact NNLO scale dependence of Ref. [9] these results are the best present estimates for the hadro-production cross section of top-quark pairs. We conclude in Sec. 4 and give some relevant formulae to the Appendix. In addition cross sections predictions using different approximations for individual PDFs are also listed in the Appendix.

## 2 Theory status

Throughout this article, we restrict ourselves to the inclusive hadronic cross section (see e.g. Ref. [20] for recent work on top-quark pair invariant mass distributions). Denoting the hadronic center-of-mass energy squared by and the top-quark mass by the total hadronic cross section for top-quark pair production is obtained through

(1) |

The parton luminosities are defined through

(2) |

where is the PDF describing the density of partons of flavor in the proton carrying a fraction of the initial proton momentum, at factorization scale . Note that we have included into the definition of to allow an easy comparison of the luminosity function between different colliders, in particular LHC and Tevatron. The sum in Eq. (1) runs over all massless parton flavors and the top-quark mass used is the so-called pole mass.

Within the context of perturbative QCD the standard way to estimate the theoretical uncertainty for the inclusive hadronic cross section in Eq. (1) is based on the residual dependence on the factorization/renormalization scale . Starting from the available predictions to a certain order in perturbation theory it is common practice to identify the factorization scale with the renormalization scale (i.e. ) and to estimate the effect of uncalculated higher orders by varying in the interval . For a given global PDF fit in contrast, the uncertainties which stem from uncertainties of the experimental data used in the fits are treated systematically by a family of pairs of PDFs, where is the number of parameters used in the fit. Then, the systematic uncertainty for the observable under consideration is estimated by (e.g. [21, 11]),

(3) |

Here the observable are obtained by using the parton distribution functions obtained by a “statistical” -variation of the th fit parameter after diagonalization of the correlation matrix. (Strictly speaking the fit parameters are varied by an amount which the authors of the corresponding PDF set take to be equivalent to a -variation.) To end up with an estimate of the overall uncertainty the uncertainty coming from the PDFs has to be combined with the uncertainty due to uncalculated higher orders. Given that the two uncertainties are very different from each other: in one case we are faced with the traces of an experimental uncertainty—in the other case we have the systematic uncertainty due to missing higher order corrections which clearly do not follow any statistical law. Adding in quadrature the two uncertainties therefore seems to be inappropriate and we use a linear combination of the uncertainties as a conservative estimate for the total uncertainty of the top-quark pair cross-section:

(4) |

where is computed according to Eq. (3). The NLO QCD corrections for the partonic cross sections in Eq. (1) (known since long time [4, 5, 6]) provide the first instance in this procedure where a meaningful error can be defined through Eq. (4).

Thus, let us start our discussion of the various theoretical uncertainties by reviewing at NLO in QCD some basic aspects concerning the parton luminosities as defined in Eq. (2) at LHC (Fig. 1) and Tevatron (Fig. 2). At LHC the highest flux is provided by the quark-gluon initial state (first plot of Fig. 1). However, as can be seen from the cross section plot of Fig. 1, the parton level cross section is much smaller than for the - or -initiated processes, since the -channel is of order and thus formally a NLO correction. As a consequence, in the total hadronic cross section the -channel gives only a contribution at the percent level (see second last plot in Fig. 1). In principle the same argument applies for -channel, however its contribution to the hadronic cross section is even further suppressed because of the smaller parton luminosity.

The second largest parton flux is delivered by the -channel. In combination with the large partonic cross section this is the most important channel at LHC, resulting in about 90% of all top-quark pairs produced via gluon fusion. Close to threshold the uncertainty of the gluon flux (estimated using Eq. 3, see also discussion there) is about 3% and at TeV it grows to almost 10%. However, given that the -channel is largely saturated at parton energies TeV, the large PDF uncertainty above TeV does not have significant impact on the overall uncertainty of in Eq. (1), see last plot in Fig. 1.

The parton luminosity ranks third at LHC. Close to threshold the -flux is suppressed by roughly a factor 10 compared to . The corresponding parton cross section vanishes in the high energy limit in contrast to the - and -case where the partonic cross sections approach a constant at high energies. Thus, the -contribution to the hadronic cross section saturates well below TeV and adds the known 10% at LHC. Due to the small numerical contribution of the - and -channels the PDF uncertainty of the hadronic cross section is entirely dominated by the uncertainty of .

At Tevatron, the situation is reversed (see Fig. 2). The luminosities are ordered in magnitude according to . This makes the -channel by far the dominant one contributing 85% to the hadronic cross section , while gluon fusion almost makes up for the rest. Although the PDF uncertainty of the -flux are only 3–4% at low energies the overall PDF uncertainty of the top-quark cross section is large, because of the sensitivity to the gluon PDF content at large-, which is still poorly constrained at present (see Fig. 2).

Finally, it is interesting to determine the value of for which the cross section

(5) |

saturates the total cross section to . At Tevatron this happens at GeV as can be seen from Fig. 2. Thus, the total cross section is largely dominated by parton kinematics in the range close to the threshold of the top-quark pair. This makes top-quark pair production at Tevatron an ideal place to apply threshold resummation. At LHC energies in contrast, the available phase space is larger and saturation to is only reached at parton energies TeV (see Fig. 1). This makes the cross section less sensitive to Sudakov logarithms, although numerically a significant part still originates from the threshold region for parton kinematics due to the steeply decreasing parton fluxes.

Further refinements of perturbative predictions for in Eq. (1) do rely on subsequent higher orders to be calculated. In particular, the knowledge about large logarithmic corrections from regions of phase space near partonic threshold allows for improvements of the theoretical accuracy beyond NLO in QCD. These Sudakov type corrections can be organized to all orders by means of a threshold resummation (e.g. to NLL accuracy [7, 8]), which has been the basis for phenomenological predictions employing a resummed cross section as defined in Ref. [8] (and also used in Ref. [14]).

However, before updating the NLL resummed results of Ref. [8] let us briefly give some relevant resummation formulae. It is well known that soft gluon resummation for -production relies on a decomposition of the parton-level total cross-section in the color basis, conveniently defined by color-singlet and color-octet final states. Then we can decompose

(6) |

Moreover, we use the standard definition of Mellin moments

(7) |

with

(8) |

Then, the resummed Mellin-space cross sections (defined in the -scheme) for the individual color structures of the scattering process are given by a single exponential (see e.g. Refs. [22, 23]),

(9) |

where denotes the Born term and the exponents are commonly expressed as

(10) |

where and . To NLL accuracy the (universal) functions as well as the functions are relevant in Eq. (10), of course, together with the appropriate matching functions in Eq. (9). Explicit expressions can be found below.

For phenomenological applications [8] the soft-gluon resummation in -space at the parton level one introduces an improved (resummed) cross section , which is obtained by an inverse Mellin transformation as follows,

(11) | |||||

where is the standard fixed order cross section at NLO in QCD and is the perturbative truncation of Eq. (9) at the same order in . Thus, the right-hand side of Eq. (11) reproduces the fixed order results and resums soft-gluon effects beyond NLO to NLL accuracy.

In Fig. 3 we plot the resummed cross section as defined in Eq. (11) zooming in on the threshold region. We display the -channel (left) and the -channel (right) as a function of the distance from the partonic threshold at . As mentioned already the -channel is suppressed by an additional power of and therefore does not contribute large Sudakov logarithms to the accuracy considered here.

The results for as shown in Fig. 3 have been obtained by performing the inverse Mellin transform in Eq. (11) numerically. Following the procedure described in Ref. [8] we have compared our results obtained from the numerical inversion with the ones shown in Ref. [8] and found complete agreement. To be precise, the treatment of the constant terms in Ref. [8] (i.e. the terms denoted in Eq. (9)) differs slightly from the minimal approach, e.g. Eq. (11). Some constants which are formally subleading have been included in Ref. [8], and moreover, several schemes for power suppressed terms in have been implemented. The resummed result shown in Fig. 3 is defined through Eq. (63) of Ref. [8] with the parameter set to 2. Another issue concerns the precise numerical matching of the exact NLO cross section and the resummed result in Eq. (11). We apply the resummed result only for GeV. The exact point is determined from the crossing of the two curves for and . Note that the precise numerical value is not important. Effectively is thereby restricted to a region of parton energies of or in other words, to a kinetic energy of one top-quark of a few GeV.

only scale uncertainty | only pdf uncertainty | total uncertainty | |||||||

m | min | max | min | max | min | max | |||

165 | 8.29 | 9.41 | 7 | 8.58 | 9.61 | 6 | 7.86 | 9.99 | 12 |

166 | 8.03 | 9.11 | 7 | 8.31 | 9.3 | 6 | 7.61 | 9.67 | 12 |

167 | 7.78 | 8.83 | 7 | 8.06 | 9.01 | 6 | 7.38 | 9.37 | 12 |

168 | 7.54 | 8.55 | 7 | 7.81 | 8.73 | 6 | 7.15 | 9.07 | 12 |

169 | 7.31 | 8.28 | 7 | 7.57 | 8.46 | 6 | 6.93 | 8.79 | 12 |

170 | 7.09 | 8.03 | 7 | 7.34 | 8.2 | 6 | 6.72 | 8.51 | 12 |

171 | 6.87 | 7.78 | 7 | 7.12 | 7.94 | 6 | 6.52 | 8.25 | 12 |

172 | 6.66 | 7.54 | 7 | 6.9 | 7.7 | 6 | 6.32 | 7.99 | 12 |

173 | 6.46 | 7.31 | 7 | 6.69 | 7.46 | 6 | 6.13 | 7.75 | 12 |

174 | 6.26 | 7.09 | 7 | 6.49 | 7.23 | 6 | 5.94 | 7.51 | 12 |

175 | 6.07 | 6.87 | 7 | 6.3 | 7.01 | 6 | 5.77 | 7.28 | 12 |

176 | 5.89 | 6.67 | 7 | 6.11 | 6.8 | 6 | 5.59 | 7.06 | 12 |

177 | 5.71 | 6.47 | 7 | 5.93 | 6.59 | 6 | 5.43 | 6.84 | 12 |

178 | 5.54 | 6.27 | 7 | 5.75 | 6.4 | 6 | 5.26 | 6.64 | 12 |

179 | 5.38 | 6.08 | 7 | 5.58 | 6.2 | 6 | 5.11 | 6.44 | 12 |

180 | 5.22 | 5.9 | 7 | 5.41 | 6.02 | 6 | 4.96 | 6.24 | 12 |

only scale uncertainty | only pdf uncertainty | total uncertainty | |||||||

m | min | max | min | max | min | max | |||

165 | 8.53 | 9.87 | 8 | 9.19 | 9.7 | 3 | 8.32 | 10.1 | 10 |

166 | 8.26 | 9.56 | 8 | 8.9 | 9.38 | 3 | 8.05 | 9.83 | 10 |

167 | 8 | 9.25 | 8 | 8.62 | 9.08 | 3 | 7.8 | 9.51 | 10 |

168 | 7.74 | 8.95 | 8 | 8.34 | 8.8 | 3 | 7.55 | 9.21 | 10 |

169 | 7.5 | 8.67 | 8 | 8.08 | 8.52 | 3 | 7.31 | 8.92 | 10 |

170 | 7.26 | 8.4 | 8 | 7.83 | 8.25 | 3 | 7.08 | 8.63 | 10 |

171 | 7.04 | 8.13 | 8 | 7.58 | 7.99 | 3 | 6.86 | 8.36 | 10 |

172 | 6.82 | 7.87 | 8 | 7.35 | 7.74 | 3 | 6.65 | 8.1 | 10 |

173 | 6.6 | 7.63 | 8 | 7.12 | 7.5 | 3 | 6.44 | 7.84 | 10 |

174 | 6.4 | 7.39 | 8 | 6.9 | 7.26 | 3 | 6.24 | 7.6 | 10 |

175 | 6.2 | 7.16 | 8 | 6.69 | 7.04 | 3 | 6.05 | 7.36 | 10 |

176 | 6.01 | 6.94 | 8 | 6.48 | 6.82 | 3 | 5.87 | 7.13 | 10 |

177 | 5.83 | 6.73 | 8 | 6.28 | 6.61 | 3 | 5.69 | 6.91 | 10 |

178 | 5.65 | 6.52 | 8 | 6.09 | 6.41 | 3 | 5.51 | 6.7 | 10 |

179 | 5.48 | 6.32 | 8 | 5.9 | 6.21 | 3 | 5.35 | 6.49 | 10 |

180 | 5.31 | 6.13 | 8 | 5.72 | 6.02 | 3 | 5.18 | 6.29 | 10 |

only scale uncertainty | only pdf uncertainty | total uncertainty | |||||||

m | min | max | min | max | min | max | |||

165 | 937 | 1154 | 11 | 1006 | 1074 | 4 | 906 | 1191 | 14 |

166 | 911 | 1122 | 11 | 978 | 1044 | 4 | 881 | 1159 | 14 |

167 | 886 | 1091 | 11 | 951 | 1016 | 4 | 856 | 1127 | 14 |

168 | 862 | 1061 | 11 | 925 | 988 | 4 | 833 | 1096 | 14 |

169 | 838 | 1032 | 11 | 900 | 962 | 4 | 810 | 1066 | 14 |

170 | 816 | 1004 | 11 | 875 | 936 | 4 | 788 | 1038 | 14 |

171 | 794 | 977 | 11 | 852 | 911 | 4 | 767 | 1010 | 14 |

172 | 773 | 950 | 11 | 829 | 887 | 4 | 746 | 983 | 14 |

173 | 752 | 925 | 11 | 806 | 863 | 4 | 726 | 957 | 14 |

174 | 732 | 900 | 11 | 785 | 841 | 4 | 707 | 931 | 14 |

175 | 713 | 877 | 11 | 764 | 819 | 4 | 688 | 907 | 14 |

176 | 694 | 853 | 11 | 744 | 797 | 4 | 670 | 883 | 14 |

177 | 676 | 831 | 11 | 724 | 777 | 4 | 653 | 860 | 14 |

178 | 659 | 809 | 11 | 705 | 757 | 4 | 636 | 838 | 14 |

179 | 642 | 788 | 11 | 687 | 737 | 4 | 619 | 816 | 14 |

180 | 625 | 768 | 11 | 669 | 718 | 4 | 603 | 795 | 14 |

only scale uncertainty | only pdf uncertainty | total uncertainty | |||||||

m | min | max | min | max | min | max | |||

165 | 986 | 1222 | 11 | 1084 | 1110 | 2 | 974 | 1236 | 12 |

166 | 959 | 1189 | 11 | 1054 | 1080 | 2 | 947 | 1203 | 12 |

167 | 933 | 1156 | 11 | 1026 | 1050 | 2 | 921 | 1170 | 12 |

168 | 908 | 1125 | 11 | 998 | 1022 | 2 | 896 | 1138 | 12 |

169 | 883 | 1094 | 11 | 971 | 995 | 2 | 872 | 1108 | 12 |

170 | 860 | 1065 | 11 | 945 | 968 | 2 | 849 | 1078 | 12 |

171 | 837 | 1036 | 11 | 920 | 943 | 2 | 826 | 1049 | 12 |

172 | 815 | 1009 | 11 | 895 | 918 | 2 | 804 | 1021 | 12 |

173 | 793 | 982 | 11 | 872 | 894 | 2 | 783 | 994 | 12 |

174 | 773 | 956 | 11 | 849 | 870 | 2 | 763 | 968 | 12 |

175 | 753 | 931 | 11 | 827 | 848 | 2 | 743 | 943 | 12 |

176 | 733 | 907 | 11 | 805 | 826 | 2 | 723 | 918 | 12 |

177 | 714 | 883 | 11 | 784 | 805 | 2 | 705 | 895 | 12 |

178 | 696 | 860 | 11 | 764 | 784 | 2 | 686 | 872 | 12 |

179 | 678 | 838 | 11 | 744 | 764 | 2 | 669 | 849 | 12 |

180 | 661 | 817 | 11 | 725 | 745 | 2 | 652 | 828 | 12 |

It should be stressed, that the total hadronic cross section is not very sensitive to these fine details due to the convolution with the parton luminosities in Eq. (1). However, to per mille accuracy (see Tabs. 1–4) these details become noticeable. Having them clarified, we are now in a position to update previous results [8, 14] for the -cross section using modern PDFs, such as the CTEQ6.5 PDF set [24]. In comparison to older sets, we find e.g. a shift of 3% in the total cross section between the PDF sets CTEQ6.5 [24] and CTEQ6.1 [21], see also Ref. [11]. Since Eq. (11) effectively contains the dominant part of higher orders (NNLO and beyond) it seems however equally appropriate to use also the MRST-2006 NNLO PDF set [25]. From the results in Tabs. 1–4 and Fig. 4 we conclude that the present overall uncertainty on the NLL resummed -cross section is 12% at Tevatron with a small shift of the central value between different PDF sets. At LHC the NLL resummed cross section of Ref. [8] reduces effectively to the NLO QCD prediction of Refs. [4, 5] with an overall uncertainty of 14%. This is due to the small gluon contribution close to threshold (see Fig. 3) and the cut when matching NLO and the in the numerical determinations. Thus the reduction of the theoretical uncertainty through Eq. (11) is marginal in this case. We will see in the next Section 3, how this situation can be improved with the help of approximate NNLO QCD corrections.

## 3 Prospects at NNLO in QCD

Let us now extend the theory predictions for heavy-quark hadro-production. We will focus on the threshold region and improve soft gluon resummation to NNLL accuracy. Subsequently, we employ the resummed cross section to generate higher order perturbative corrections – more specifically an approximate NNLO cross section which is exact to logarithmic accuracy (including the Coulomb corrections). To that end, we briefly recall the steps leading to the final form for in Eq. (10). In order to achieve NNLL accuracy the function is of particular interest here.

The exponential in Eq. (9) is build up from universal radiative factors for the individual color structures which take the form

(12) |

where the exponentiation of singlet contribution (i.e. a colorless massive final state) follows from the Drell-Yan process and hadronic Higgs production in gluon fusion. The corresponding functions and are very well-known [26, 27, 28]. The exponentiation of the color-octet contribution receives an additional contribution due to soft gluon emission from the heavy-quark pair in the final state. The final-state system carries a total color charge given by the charge, thus its contribution to soft radiation vanishes in the color-singlet channels regardless of the initial state partons. Moreover gluon emission from massive quarks does not lead to collinear logarithms and therefore starts at NLL accuracy only. Explicit formulae are

(13) | |||||

(14) |

with anomalous dimensions and , corresponding to DY and Higgs, respectively. The effects of collinear soft-gluon radiation off initial-state partons are collected by the first term in Eq. (13) while the process-dependent contributions from large-angle soft gluons are resummed by the second term. Soft radiation from the heavy-quark pair in the final state is summarized by in Eq. (14) with the corresponding anomalous dimension .

The extension to NNLL requires the and to three loops [29, 30] and the function and to two loops [26, 27, 28] (the latter are actually known to three loops as well [31, 32]). Explicit expressions using the expansions

(15) |

are collected in Eqs. (A)–(A.4) in the Appendix. The remaining anomalous dimensions for soft radiation off a heavy-quark pair in the final state is needed to two loops. For the latter we use the exact calculation of the two-loop QCD corrections to the massive heavy quark form factor [33] along with Ref. [34], where the exponentiation of the form factor for massive colored particles in the limit has been clarified. From the all-order singularity structure of the massive form factor [34], we can read off the single poles corresponding to soft gluon emission at one and two loops. After a trivial substitution of color factors ( for ) we find

(16) |

As pointed out in Ref. [8] the one-loop value of agrees with Ref. [7] where the soft anomalous dimension matrix (in color space) for heavy-quark production has been calculated at order . In the limit the matrix diagonalizes in the singlet-octet basis and reproduces from its eigenvalue in the octet channel. Moreover, the structure of as determined from Ref. [34] agrees also with the two-loop soft anomalous dimension matrix for vanishing parton masses which obeys the following factorization property [35, 36],

(17) |

with the well-known ratio [37]. As a further check on Eq. (16) it would, of course, be very interesting to repeat the calculation of Ref. [35, 36] for heavy-quark hadro-production at two loops, i.e. with non-vanishing parton masses .

Finally, explicit integration of Eqs. (13)–(14) leads to the functions , , of Eq. (10) and to the matching in Eq. (9) which we collected in Eqs. (A.5)–(A.13) in the Appendix. All formulae can be obtained by simple substitutions e.g. from deep-inelastic scattering (DIS) in Ref. [28]. In Fig. 5 we display the resummed cross section of Eq. (9) (normalized to the respective Born result) for the and the -channel in increasing logarithmic accuracy. Fig. 5 clearly shows the good convergence property of the NNLL contribution similar to other observables investigated previously [26, 27, 28]. As a matter of fact, Eq. (10) may even be extended to next-to-next-to-next-to-leading accuracy (NLL), as the relevant functions can be easily derived from Ref. [28] and the respective anomalous dimensions are known. Following the arguments based on the exponentiation of the form factor for massive colored partons [34] leading to Eq. (16) we identify and for the four-loop terms and a Padé estimate exists [28]. However, presently we are lacking knowledge on the matching functions at this order. From experience we expect NLL effects to be numerically very small, though, and we leave this issue to future investigations.

Let us instead use the resummed cross section (now known at NNLL accuracy) to construct an approximate NNLO cross section by expanding Eq. (9) to second order. In this way, we determine the corresponding Sudakov logarithms appearing in the NNLO corrections, i.e. the powers of in Mellin space or in momentum space with and the velocity of the heavy quark

As a technical remark, we stress here that in a fixed order expansion the inverse Mellin transformation, i.e. the mapping of powers of to powers of can be uniquely performed. The Mellin-space accuracy up to power suppressed terms in corresponds to neglecting higher order polynomials in with . We give some formulae in the Appendix. Moreover, we can even include the complete Coulomb corrections at two loops thanks to Ref. [33, 38]. In the singlet-octet decomposition of the individual color structures in the cross section, the result of Ref. [33, 38] can be directly applied to the singlet case, while a simple modification of the color factors (that is instead of ) accounts for the octet case (see e.g. [39]).

Thus, we are in a position to present the threshold expansion of the inclusive partonic cross sections entering Eq. (1). In the perturbative expansions in powers of the strong coupling constant as defined in Eq. (15) and setting and , we have for the channel in the -scheme

(18) | |||||

(19) | |||||

(20) | |||||

(21) | |||||

The terms proportional to inverse powers of correspond to the Coulomb corrections and the presently unknown two-loop constants and are set to zero. For reference, we have also repeated the well-known NLO results Eq. (18) and Eq. (20). The lengthy analytical results (containing the explicit dependence on the color factors and on ) are given in the Appendix, Eqs. (A.17)–(A.20). We define a NNLO (approx) cross section to be used in this paper as the sum of exact NLO result and the two-loop contribution of Eqs. (19) and (21) for all scale independent terms. All scale dependent terms at NNLO accuracy are long known exactly [9] as they can be easily constructed from the lower orders convoluted with the appropriate splitting functions. We use the exact result of Ref. [9] for the -dependence at two loops. As emphasized several times, the - and -contributions are small at Tevatron and LHC and we simply keep them at NLO here.

In Fig. 6 we display the NNLO (approx) results for the partonic cross sections as calculated in Eqs. (19) and (21). We plot (left) and (right) again as a function of the distance from threshold at (solid lines in Fig. 6). This is useful to asses the question what improvements can be expected from a full NNLO calculation. Given that the -factor of the NLO result is of moderate size at large partonic energies one can expect that the full NNLO corrections should give only small corrections in this region of phase space. On the other hand the -factor of the NLO correction becomes large in the threshold region (i.e. GeV), where finally perturbation theory breaks down. In this region the corrections are dominated by the large logarithms in together with the Coulomb corrections which are correctly described by Eqs. (19) and (21). In other words, where we expect large corrections from the full NNLO QCD calculation our should provide a good estimate. This is further supported by Ref. [15] where the next-to-leading order corrections to top-quark pair production together with an additional jet have been calculated. This contribution represents part of the NNLO corrections for inclusive top-quark pair production. In Ref. [15] it was found that for the NLO corrections to production are almost zero. This is a further indication that the hard corrections to the inclusive top-quark pair production at NNLO are indeed small. Moreover, as mentioned above, we have further improved by incorporating the complete scale dependence at NNLO which is already known exactly [9]. To that end let us quantify in detail once more the range of validity for the soft gluon approximations. We show in Tab. 5 the numerical size of the individual logarithms and powers in in Eqs. (18)–(21) when evaluated at a given parton energy . As a consequence of the moderate size of the expansion coefficients in Eqs. (18)–(21), we clearly see the good convergence properties of the logarithmic expansion up energies GeV. Beyond that value the soft logarithms (being proportional to the Born cross section) smoothly vanish.

[GeV] | |||||||
---|---|---|---|---|---|---|---|

0.1 | 191.9844 | -51.5762 | 13.8558 | -3.7223 | 1710.7500 | 41.3612 | 0.0242 |

0.5 | 72.5503 | -24.8588 | 8.5176 | -2.9185 | 342.7502 | 18.5135 | 0.0540 |

1.0 | 43.8302 | -17.0345 | 6.6204 | -2.5730 | 171.7504 | 13.1054 | 0.0763 |

5.0 | 9.9709 | -5.6111 | 3.1577 | -1.7770 | 34.9518 | 5.9120 | 0.1691 |

10.0 | 4.3130 | -2.9928 | 2.0768 | -1.4411 | 17.8536 | 4.2254 | 0.2367 |

50.0 | 0.2628 | -0.3671 | 0.5127 | -0.7160 | 4.1870 | 2.0462 | 0.4887 |

100.0 | 0.0434 | -0.0951 | 0.2084 | -0.4565 | 2.4919 | 1.5786 | 0.6335 |

500.0 | 0.0001 | -0.0007 | 0.0081 | -0.0901 | 1.1976 | 1.0943 | 0.9138 |

In addition we show in Fig. 6 also previous approximations to the NNLO correction from Ref. [9] (dashed lines) employing two distinct differential kinematics to define the partonic threshold. They agree with our NNLO (approx) corrections for GeV if Eqs. (19) and (21) are truncated to the first three powers in . However, at higher partonic center-of-mass energies the results of Ref. [9] receive large numerical contributions from sub-leading terms and become unreliable (see in particular Fig. 6 on the right).

We would also like to point out that there is a discrepancy between the NLL resummed cross section of Ref. [8] and Eq. (11) and the fixed order NNLO approximation discussed here. In particular for the gluon fusion channel in Fig. 3 (right) and Fig. 6 (right) the numerical differences between and are rather large. The all-order NLL resummed cross section is significantly smaller than its expansion to second-order Eq. (21) or the corresponding result of Ref. [9], the latter two both being consistent with each other. We can attribute this difference to the following fact: For -hadro-production the Born cross section exhibits simple (although non-trivial) -dependence and the resummed cross section in Mellin space (as implemented in Ref. [8] and Eq. (11)) contains products of -dependent functions. This is unlike other cases considered in the literature, where the Born terms have always been proportional to a delta-function, i.e. for DIS, Drell-Yan or Higgs production. In momentum space products of -dependent functions correspond to convolutions, which induce formally sub-leading but numerically large corrections in the resummed result. Eventually, this leads to the observed suppression in Fig. 3. Most likely this large discrepancy will also persist when comparing to a full NNLO QCD calculation, or upon matching the latter to a resummed cross section at NNLL accuracy along the lines of Eq. (11). This fact has to be kept in mind when using for predictions at LHC, where the -channel dominates. As mentioned above, for any finite order expansion in , there is no ambiguity in performing the inverse Mellin transformation analytically up to power suppressed terms in or, equivalently in .

We are now in a position to present the new results for the top-quark cross section at NNLO (approx) as defined below Eq. (21) including the exact scale dependence. We also quote the corresponding uncertainty according to Eq. (4). In our study we use the same PDFs as in Tabs. 1–4 above.

In Fig.7 the scale dependence for and is shown. For the we use the PDF set MRST-2006 NNLO while for the PDF set CTEQ6.5 is used. To become less sensitive to different normalizations we normalise the curves to the central value . In addition we show also the results obtained by using the Alekhin PDF set [40] available in NLO and NNLO accuracy. After normalisation one can see that the two curves for the NLO predictions agree rather well as one might expect. For the two NNLO curves the agreement is less good in particular for extreme values of the scale. The origin of the minor discrepancy might be attributed to slightly different input densities at low scale. Compared to the NLO results the scale dependence of is improved. In particular we find a plateau at . Note that due to the different shape of the NNLO curve the uncertainty estimate of Eq. (4) has to be adapted here. Restricting the scale to the interval the residual scale dependence of is reduced to a few percent.

In Fig. 8 we plot the total cross section at Tevatron and display also CDF data [41] with GeV. The corresponding cross section values are given in Tabs. 6 and 7. By using the residual scale dependence is reduced to 3%. Compared to and presented in the previous section this corresponds to a reduction by a factor of 2. The data points nicely agree with the theoretical prediction. The overall uncertainty of the the theoretical prediction is about 8% for CTEQ6.5 and 6% for MRST-2006 NNLO — an accuracy unlikely to be reached at the Tevatron experiments. Note that the smaller PDF uncertainty obtained when using the MRST-2006 NNLO PDF set is due to a different convention used by the MRST collaboration to define the PDF uncertainty. In Fig. 9 (right) we show for the LHC. Again we observe a drastic reduction of the scale uncertainty compared to and . For comparison we show also in Fig. 9 (left). The corresponding cross section values are listed in Tabs. 8 and 9. Apart from reducing the scale dependence the leads only to a small shift of a few percent in the central value for the cross section prediction. The band is well contained in the band. So perturbation theory seems to be well behaved and under control. The overall uncertainty is about 6% for the CTEQ6.5 PDF set and about 4% for the MRST-2006 NNLO set.

The numbers quoted in Tabs. 6–9 represent presently the best estimates for the top-quark production cross section at Tevatron and LHC (see the Appendix for additional information on the individual PDFs and their eigenvalues). It should be kept in mind, though, that there is an intrinsic uncertainty in the central value at of our NNLO (approx) result due to neglected power corrections in away from threshold. However, due to the steeply falling parton flux (see Figs. 1, 2), the numerical impact of these contributions is much suppressed.

only scale uncertainty | only pdf uncertainty | total uncertainty | |||||||

m | min | max | min | max | min | max | |||

165 | 9.26 | 9.66 | 3 | 9.04 | 10.1 | 6 | 8.73 | 10.1 | 8 |

166 | 8.97 | 9.36 | 3 | 8.76 | 9.82 | 6 | 8.46 | 9.87 | 8 |

167 | 8.68 | 9.07 | 3 | 8.49 | 9.51 | 6 | 8.2 | 9.57 | 8 |

168 | 8.41 | 8.79 | 3 | 8.22 | 9.22 | 6 | 7.94 | 9.27 | 8 |

169 | 8.15 | 8.52 | 3 | 7.97 | 8.93 | 6 | 7.7 | 8.98 | 8 |

170 | 7.9 | 8.26 | 3 | 7.73 | 8.65 | 6 | 7.46 | 8.7 | 8 |

171 | 7.65 | 8.01 | 3 | 7.49 | 8.38 | 6 | 7.23 | 8.44 | 8 |

172 | 7.42 | 7.76 | 3 | 7.26 | 8.12 | 6 | 7.01 | 8.18 | 8 |

173 | 7.19 | 7.53 | 3 | 7.04 | 7.87 | 6 | 6.8 | 7.93 | 8 |

174 | 6.97 | 7.3 | 3 | 6.83 | 7.63 | 6 | 6.59 | 7.69 | 8 |

175 | 6.76 | 7.08 | 3 | 6.62 | 7.4 | 6 | 6.39 | 7.45 | 8 |

176 | 6.55 | 6.87 | 3 | 6.43 | 7.17 | 6 | 6.2 | 7.23 | 8 |

177 | 6.36 | 6.66 | 3 | 6.23 | 6.96 | 6 | 6.01 | 7.01 | 8 |

178 | 6.16 | 6.46 | 3 | 6.05 | 6.75 | 6 | 5.83 | 6.8 | 8 |

179 | 5.98 | 6.27 | 3 | 5.87 | 6.54 | 6 | 5.66 | 6.6 | 8 |

180 | 5.8 | 6.08 | 3 | 5.69 | 6.35 | 6 | 5.49 | 6.4 | 8 |

only scale uncertainty | only pdf uncertainty | total uncertainty | |||||||

m | min | max | min | max | min | max | |||

165 | 9.59 | 10 | 3 | 9.73 | 10.2 | 3 | 9.34 | 10.3 | 6 |

166 | 9.28 | 9.76 | 3 | 9.42 | 9.94 | 3 | 9.04 | 10 | 6 |

167 | 8.99 | 9.45 | 3 | 9.12 | 9.62 | 3 | 8.75 | 9.7 | 6 |

168 | 8.7 | 9.16 | 3 | 8.83 | 9.31 | 3 | 8.47 | 9.39 | 6 |

169 | 8.42 | 8.87 | 3 | 8.55 | 9.02 | 3 | 8.2 | 9.1 | 6 |

170 | 8.16 | 8.59 | 3 | 8.28 | 8.73 | 3 | 7.94 | 8.81 | 6 |

171 | 7.9 | 8.32 | 3 | 8.02 | 8.46 | 3 | 7.69 | 8.53 | 6 |

172 | 7.65 | 8.06 | 3 | 7.77 | 8.19 | 3 | 7.45 | 8.27 | 6 |

173 | 7.41 | 7.81 | 3 | 7.53 | 7.93 | 3 | 7.22 | 8.01 | 6 |

174 | 7.18 | 7.57 | 3 | 7.29 | 7.69 | 3 | 6.99 | 7.76 | 6 |

175 | 6.95 | 7.34 | 3 | 7.07 | 7.45 | 3 | 6.77 | 7.52 | 6 |

176 | 6.74 | 7.11 | 3 | 6.85 | 7.22 | 3 | 6.57 | 7.29 | 6 |

177 | 6.53 | 6.89 | 3 | 6.64 | 6.99 | 3 | 6.36 | 7.07 | 6 |

178 | 6.33 | 6.68 | 3 | 6.43 | 6.78 | 3 | 6.17 | 6.85 | 6 |

179 | 6.13 | 6.48 | 3 | 6.24 | 6.57 | 3 | 5.98 | 6.64 | 6 |

180 | 5.95 | 6.28 | 3 | 6.05 | 6.37 | 3 | 5.8 | 6.44 | 6 |

only scale uncertainty | only pdf uncertainty | total uncertainty | |||||||

m | min | max | min | max | min | max | |||

165 | 1035 | 1082 | 3 | 1048 | 1117 | 4 | 1003 | 1117 | 6 |

166 | 1007 | 1052 | 3 | 1019 | 1086 | 4 | 975 | 1086 | 6 |

167 | 979 | 1024 | 3 | 991 | 1056 | 4 | 948 | 1056 | 6 |

168 | 953 | 996 | 3 | 964 | 1028 | 4 | 922 | 1028 | 6 |

169 | 927 | 969 | 3 | 937 | 1000 | 4 | 897 | 1000 | 6 |

170 | 902 | 943 | 3 | 912 | 973 | 4 | 873 | 973 | 6 |

171 | 878 | 917 | 3 | 887 | 947 | 4 | 849 | 947 | 6 |

172 | 855 | 893 | 3 | 863 | 922 | 4 | 827 | 922 | 6 |

173 | 832 | 869 | 3 | 840 | 898 | 4 | 805 | 898 | 6 |

174 | 810 | 846 | 3 | 818 | 874 | 4 | 783 | 874 | 6 |

175 | 789 | 824 | 3 | 796 | 851 | 4 | 762 | 851 | 6 |

176 | 768 | 802 | 3 | 775 | 829 | 4 | 742 | 829 | 6 |

177 | 748 | 781 | 3 | 755 | 808 | 4 | 723 | 808 | 6 |

178 | 729 | 761 | 3 | 735 | 787 | 4 | 704 | 787 | 6 |

179 | 710 | 741 | 3 | 716 | 767 | 4 | 686 | 767 | 6 |

180 | 692 | 722 | 3 | 698 | 747 | 4 | 668 | 747 | 6 |

only scale uncertainty | only pdf uncertainty | total uncertainty | |||||||

m | min | max | min | max | min | max | |||

165 | 1094 | 1141 | 3 | 1128 | 1154 | 2 | 1082 | 1154 | 4 |

166 | 1064 | 1110 | 3 | 1097 | 1122 | 2 | 1052 | 1122 | 4 |

167 | 1035 | 1080 | 3 | 1067 | 1092 | 2 | 1024 | 1092 | 4 |

168 | 1008 | 1050 | 3 | 1038 | 1063 | 2 | 996 | 1063 | 4 |

169 | 981 | 1022 | 3 | 1010 | 1034 | 2 | 969 | 1034 | 4 |

170 | 955 | 995 | 3 | 983 | 1007 | 2 | 943 | 1007 | 4 |

171 | 929 | 969 | 3 | 957 | 980 | 2 | 918 | 980 | 4 |

172 | 905 | 943 | 3 | 932 | 954 | 2 | 894 | 954 | 4 |

173 | 881 | 918 | 3 | 907 | 929 | 2 | 871 | 929 | 4 |

174 | 858 | 894 | 3 | 883 | 905 | 2 | 848 | 905 | 4 |

175 | 836 | 871 | 3 | 860 | 882 | 2 | 826 | 882 | 4 |

176 | 814 | 848 | 3 | 838 | 859 | 2 | 804 | 859 | 4 |

177 | 793 | 826 | 3 | 816 | 837 | 2 | 783 | 837 | 4 |

178 | 773 | 805 | 3 | 795 | 815 | 2 | 763 | 815 | 4 |

179 | 753 | 785 | 3 | 775 | 795 | 2 | 744 | 795 | 4 |

180 | 734 | 765 | 3 | 755 | 774 | 2 | 725 | 774 | 4 |

## 4 Conclusions

In this article we have summarized the present knowledge on theory predictions for the top-quark pair production cross section at Tevatron and LHC. We have taken some care to quantify the sensitivity of the total cross section to soft gluon emission and large Sudakov type logarithms. As is well known, top-quark pair production at Tevatron is largely dominated by parton kinematics close to threshold, thus approximations based on soft gluon resummation should provide an excellent description. At LHC we find that soft gluon emission near threshold is less dominant, but contributes still a numerically sizable fraction to the total cross section. Thus, soft gluon effects in -production are still rather prominent at LHC as well.

We have updated the NLL resummed cross section as defined in Ref. [8, 14] using recent PDFs. Furthermore, we have extended the resummed predictions to NNLL accuracy and we have derived approximate NNLO cross sections which are exact to all powers in at two loops. Together with the exact NNLO scale dependence (and including the two-loop Coulomb corrections) our result for represents the best present estimate for hadro-production of top-quark pairs, both at Tevatron and LHC. As mentioned earlier we believe that hard corrections at the NNLO level are small. This is supported by the explicit findings of Ref. [15]. We have found for the NNLL resummed cross section and the finite order expansion good apparent convergence properties. Moreover, the stability of the total cross section with respect to scale variations is much improved by our NNLO (approx) result.

In closing let us briefly comment on ideas to use top-quark pair production as an additional calibration process for the parton luminosity at LHC [11]. This could become feasible because the PDF dependence of -production at LHC is anti-correlated with -boson production (the standard candle process at LHC, see e.g. [42, 43]) and correlated with Higgs boson production, especially for larger Higgs masses. It has been noted however, that the NLO theory predictions to the top-quark cross section are not accurate enough. We are confident that the NNLO (approx) results of this present paper provide a step in the right direction by further constraining the theory uncertainties for this important process.

The complete NNLO QCD predictions for heavy-quark hadro-production do not only require the hard scattering cross section but also the evolution of the parton densities to be performed at the same order employing the NNLO splitting functions [29, 30]. In addition we remark, that the present accuracy on the gluon PDF in the medium range of interest for top-quark production at LHC is well constrained by from DIS data for structure functions in -scattering from HERA and evolution, leading to the rather small uncertainty of 3% (see Fig. 1) at small energies. Thus, for top-quark pair production to become a standard candle process at LHC similar to gauge boson production and to become competitive with DIS data also an experimental accuracy much better than the currently quoted [1] value of 10% will be needed.

### Acknowledgements

We would like to thank S. Alekhin, W. Bernreuther, and E. Laenen for stimulating discussions. S.M. is supported by the Helmholtz Gemeinschaft under contract VH-NG-105 and P.U. is a Heisenberg fellow of Deutsche Forschungsgemeinschaft (DFG). This work is also partly supported by DFG in SFB/TR 9 and the hospitality of the Galileo-Galilei Institute in Florence is gratefully acknowledged.

Note added.— Shortly after submitting the preprint version of this article, the related work [44] appeared, where a similar study has been performed. In the meantime a tuned comparison of the resummed (NLL) partonic cross section has been done and we have found good agreement, once it was taken into account that the matching for the scheme implemented in [44] is slightly different from the original Ref. [8] employed in the present article. This minor scheme dependence accounts for the observed differences in the predictions for the total cross section between [44] and this article.