Quark and gluon spin-2 form factors to two-loops in QCD

We present complete two-loop radiative corrections to the graviton-quark-antiquark form factor G∗ → q\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$ \overline{q} $\end{document} and graviton-gluon-gluon form factor G∗ → g g in SU(N) gauge theory with nf light flavours using d-dimensional regularisation to all orders in ε = d − 4. Thisisanimportantingredienttonext-to-next-to-leadingorderQCDcorrections to hadronic scattering processes in models with large extra-dimensions where Kaluza-Klein graviton modes couple to Standard Model fields. We show that these form factors obey Sudakov integro-differential equation and the resulting cusp, collinear and soft anomalous dimensions coincide with those of electroweak vector boson and gluon form factors. We also find the universal behaviour of the infrared singularities in accordance with the proposal by Catani.


Introduction
Extra dimension models are interesting scenarios to tackle the hierarchy problem. Depending on the geometry of the extra dimension(s), the two popular options are: (a) flat extra dimension model (ADD) [1][2][3] and (b) the warped extra dimension model (RS) with a large curvature [4]. In both these models, only the graviton is allowed to permeate the bulk which leads to different spectrum of spin-2 Kaluza-Klein (KK) modes in 4-dimensions. The spin-2, KK modes couple to the Standard Model (SM) particles through the energy momentum tensor of the SM. These beyond SM model scenarios could alter the SM predictions by additional virtual KK mode exchanges and real KK mode productions. Dedicated groups in both ATLAS [5][6][7] and CMS [8,9] collaborations are engaged in the analysis for extra dimension searches in various processes like di-lepton, di-photon, mono-jet, mono-photon productions etc. To put stringent bounds on the parameters of these BSM models, control on the theoretical uncertainties is essential. Renormalisation and factorisation scale dependences of a cross section to a particular order in perturbation theory give an estimate of the uncalculated higher order corrections. Presently next-to-leading order (NLO) QCD calculations have been done for di-lepton [10][11][12], di-photon [13,14] and di-electroweak gauge boson [15][16][17] productions via virtual KK modes in addition to the SM contributions. These virtual contributions have been incorporated in the AMC@NLO frame work and results to NLO+PS accuracy are now available for most of the di-final state processes [18,19]. In all these processes the factorisation scale dependence reduces substantially and in addition the NLO correction is in fact significant. For the above processes, the leading order (LO) is of the order O α 0 s , the renormalisation scale dependence starts only at NLO in QCD. To control the renormalisation scale dependence one would have to go to next-to-next-toleading order (NNLO) order.
A full NNLO QCD contribution requires the knowledge of graviton-quark-antiquark G * → qq and graviton-gluon-gluon G * → gg form factors up to two-loop level in QCD JHEP02(2014)035 in addition to double real emission and one-loop single real emission scatter processes at the parton level. Here G * denotes the virtual graviton. In this article we take the first step towards the full NNLO computation by evaluating these form factors to two-loop level in QCD by sandwiching the energy momentum tensor of the QCD part of the SM between on-shell gluon and quark states. We will also discuss the infrared (IR) structure of these form factors using Sudakov's integro-differential equation and Catani's proposal on two-loop QCD amplitudes.
In the next section, we will derive the two-loop form factors and in the section 3, we describe the infrared structure of these form factors. Finally we conclude in section 4 and the appendix contains the form factors expanded in powers of ε to desired accuracy.

Two loop form factors
We work with the following action that describes the interaction of SM fields with the KK modes of the gravity. To lowest order in κ, the KK modes couple to SM fields through energy momentum tensor of SM. Here, we restrict ourselves to QCD part of the energy momentum tensor: where T QCD µν is the energy momentum tensor of QCD [10][11][12]: In the above equation, g s is the strong coupling constant and ξ is gauge parameter in Lorenz gauge fixing condition. The peculiar feature in the above action is the appearance of the direct coupling of ghost fields (ω, ω) with KK modes [10][11][12]. We have kept track of these unphysical contributions along with those coming from gauge fixing term in order to establish the cancellation of their contributions among themselves. We have retained only light flavours in the quark sector. We compute the relevant form factors by evaluating the truncated matrix elementŝ M I of T QCD µν between on-shell gluon (I = g) and quark/anti-quark (I = q, q) states. The symbolˆhere and in the following denotes that the quantities are unrenormalised/bare. TheM I s in the color space can be expanded aŝ 3)

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where the unrenormalised coupling constantâ s =ĝ 2 s /16π 2 and the scale µ is introduced to keep g s dimensionless in dimensional regularisation and the space-time dimension is taken to be d = 4 + ε. The scale Q 2 = −q 2 − iǫ, where q is the momentum transfer. The unrenormalised coupling constantâ s is related to the renormalised one a s (µ 2 R ) by where the renormalisation constant Z(µ 2 R ) is given by with µ R -renormalisation scale, C A = N, T F = 1/2 and n f the number of active flavours. Using theM I s, the form factors are defined aŝ and the symbol · takes care of the color and spin/polarisation sums. The Feynman amplitudes that contribute to gluon and quark matrix elements of the energy momentum tensor T QCD µν at born, one-loop and two-loop levels in QCD are obtained using a computer program QGRAF [20]. We find 12 one-loop and 153 two-loop diagrams that contribute to the matrix element of energy momentum tensor if it is computed between gluon states while 4 one-loop and 54 two-loop diagrams that contribute for quark-antiquark states. We have used a set of in-house FORM [21] routines to convert the QGRAF outputs into a suitable form for further symbolic manipulations. These FORM routines not only replace the symbolic Feynman vertices, propagators by the corresponding Feynman rules but also perform Lorentz contractions, Dirac gamma matrix algebra etc. We have done all our computations in d = 4 + ε dimensions in order to regulate both ultraviolet (UV) and infrared (IR) divergences. The resulting expressions at this stage contain one and two-loop tensor and scalar integrals. Since the coupling of KK modes with the energy momentum tensor involves quadratic derivatives, we find that the rank of the tensor integrals present in our computation is larger than the rank of integrals appearing in quark and gluon form factors contributing to electroweak vector boson [22][23][24][25] and Higgs production cross sections (in the infinite top quark mass limit) [26][27][28][29] respectively.
In the past, they were computed using very different methods, that is, different techniques were employed to perform loop integrals. In [22], the method of Feynman parameterisation was used in a judicious way so that after each parametric integration one is left with an integral over the next parameter. In [23], an elegant method, advocated in [30,31], namely "integration by parts" (IBP) was used. In [24,25] the integrals were computed using dispersion techniques developed in [32] which uses the Cutkosky rules [33]. In this method, one cuts the Feynman amplitude in all possible ways to obtain the imaginary part and the real part was obtained from the imaginary part via a dispersion relation. In [26], an algorithm [34] which relates l-loop integrals with n + 1 external legs to l + 1-loop integrals JHEP02(2014)035 with n external legs was used to compute two-loop QCD corrections to gluon form factor relevant for Higgs production cross section. It maps the massless two-loop vertex functions onto massless three-loop two-point functions which are relatively easy to compute. In [27], IBP identities were used extensively to compute the gluon form factor. The gluon form factor at two-loop level in SU(N ) gauge theory with n f light flavours was computed in [29] following [32]. All these results were known only to a desired accuracy in ε, say O(ε). In [35], using IBP [30,31] and Lorentz invariance (LI) [36] identities, the authors have shown that the two-loop corrections to electroweak quark and gluon form factors can be expressed in terms of only few master integrals and have also obtained for the first time the closed form solution to one of the master integrals whose result was known only up to few orders in ε. We will closely follow this approach by [35] to achieve our task. Reduction of a large number of one and two-loop tensor integrals that appear in our computation to a few master integrals was achieved by FIRE [37], a Mathematica package, which extensively uses the IBP [30,31] and LI [36] identities implemented using Laporta algorithm [38]. Note that there are also similar packages namely AIR [39], Reduce [40,41] and most recently LiteRed [42] that can do this reduction. We used LiteRed to cross-check our results obtained using FIRE. At one-loop level, we find that the form factors depend only on one master integral and at two-loop level, there are one one-loop and three two-loop master integrals. These one-loop and two-loop master integrals are now known to all orders in ε and are given in [35]. Below we present our final results forF T,(n) I for I = g, q; n = 1, 2 in terms of these master integrals.

= 1 and
The exact results for the master integrals A i (i = {2, LO}, 3, 4, 6) can be expressed in terms of Euler Gamma functions and are available in the works on two-loop electroweak form factors [35]. The most difficult crossed two-loop master integral A 6 was solved exactly in [35]. These results are used to present the form factors to order O ε 4 and are given in the appendix. We use them to study the infrared pole structure of these farm factors in the next section. The higher order terms O(ε i ), i > 0 are also useful to perform ultraviolet renormalisation of the form factors beyond two-loop level.

Infrared divergence structure
Having obtained these form factors at two-loop level, the next step is to study the infrared pole structure of these factors in order to establish the universal behaviour of these QCD amplitudes. In the past, there have been detailed studies of quark and gluon form factors through Sudakov integro-differential equation [43][44][45][46][47], see also [29,[48][49][50][51]. Since the KK modes are colour singlet fields, the unrenormalised form factorsF T I â s , Q 2 , µ 2 , ε are expected to satisfy similar integro-differential equation that follows from the gauge as well as JHEP02(2014)035 renormalisation group (RG) invariances. In dimensional regularisation, where the constants K T,I contain all the poles in ε, and G T,I are finite as ε becomes zero. The RG invariance ofF T I gives The quantities A T,I are the cusp anomalous dimensions which are expanded as Solving these RG equations, the constants K T,I and G T,I can be obtained in powers of bare coupling constantâ s . Using these solutions, we obtain, whereL I(1) . We find that they are identical to those obtained in [52], that is, those appearing in gluon and quark form factors, confirming the universality of IR structure of these form factors. The coefficients G T,I i (ε) take the following form where again the collinear anomalous dimension B T,I i and soft anomalous dimension f T,I i are found to be identical to B I i and f I i obtained in [29,53] for quark and gluon form factors. We find that only g T,I,k i are operator dependent.

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Another independent check on our computation is done by establishing the connection between these form factors and the very successful proposal by Catani [54] (also see [55]) on one and two-loop QCD amplitudes using the universal factors I (i) I (ε) and H (i) The all order generalisation of Catani's proposal was obtained by Becher and Neubert [56] and also by Gardi and Magnea [57]. These universal factors capture all the IR poles of n-parton QCD amplitudes up to two-loop level in QCD. Following [54], we proceed by expressing the matrix elements in terms of UV renormalised ones aŝ Using the universal I I (ε) obtained by Catani, we can write down M (1) (1) I,fin (ε) and T F n f . given in [54], we obtain H (2) I : 14) The single pole coefficients thus obtained agree with the color diagonal part of eq. (12) of [56] (see also eq. (4.21) of [29] for quark and gluon form factors and [58][59][60][61] for four parton amplitudes). This serves as a check on our computation and also establishes the proposal by Catani on IR universality of QCD amplitudes with T µν insertion.

Conclusions
We present an important ingredient to the full NNLO QCD correction to graviton mediated hadronic scattering processes namely the gluon and quark form factors of energy momentum tensor of the QCD part of the SM up to two-loop level in QCD. We have used dimensional regularisation to obtain these form factors in SU(N ) gauge theory with n f light flavours. Both exact as well as expanded results in ε are presented. The higher order terms in ε of these form factors are important for the ultraviolet renormalisation of these amplitudes at three-loop level. We have shown that these form factors satisfy Sudakov integro-differential equation with same cusp A I , collinear B I and soft f I anomalous dimensions that contribute to electroweak vector boson and gluon form factors. In addition, they also show the universal behaviour of the infrared poles in ε in accordance with the proposal by Catani.
Spin-2 resonance production has been widely studied in the context of the Higgs [62] and BSM models [63]. The two-loop results presented in this paper would further reduce the theoretical uncertainties and hence improve the predictions in disentangling the various postulates. We further plan to apply these two-loop results to the TeV scale gravity models [64].