# Probing the top-Higgs coupling through the secondary lepton distributions in the associated production of the top-quark pair and Higgs boson at the LHC

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## Abstract

We complement the analysis of the anomalous top-Higgs coupling effects on the secondary lepton distributions in the associated production of the top-quark pair and Higgs boson in proton–proton collisions at the LHC of the former work by one of the present authors by taking into account the quark–antiquark production mechanism. We also present simple arguments which explain why the effects of the scalar and pseudoscalar anomalous couplings on the unpolarized cross section of the process are completely insensitive to the sign of either of them.

### Keywords

Higgs Boson Monte Carlo Differential Cross Section Gluon Fusion Anomalous Coupling## 1 Introduction

*b*-quark mass \(m_b\) are neglected. At the same time there are only 32 Feynman diagrams which contribute to the signal cross section of \(t \bar{t} H\) production, two of which are shown in Fig. 1. The remaining 30 signal diagrams are obtained from those depicted by attaching the Higgs boson line of the \(Hb\bar{b}\) vertex to the other

*t*- or \(\bar{t}\)-quark line, or interchanging the

*b*and \(\bar{b}\) quarks in Fig. 1a, b and interchanging the two gluons in Fig. 1b. The diagrams with the Higgs boson line of \(Hb\bar{b}\) vertex attached to either the

*b*- or \(\bar{b}\)-quark line are not counted here, as their contribution to the \(t \bar{t} H\) production signal is suppressed by the mass ratio \(m_b/m_t\). The effects caused by modifications of the scalar and pseudoscalar couplings of the Higgs boson to top quark were clearly visible in the \(t \bar{t} H\) production signal cross section, but they were to large degree obscured by the irreducible off-resonance background.

The other signal diagrams can be obtained by attaching the Higgs boson line of the \(Hb \bar{b}\) vertex to the other *t*- or \(\bar{t}\)-quark line or interchanging the *b*- and \(\bar{b}\)-quark lines in the diagrams of Fig. 2. Let us note that another 24 diagrams which contain the Feynman propagators of the *t*-, \(\bar{t}\)-quark and the Higgs boson at a time can be obtained from the signal diagrams just described by the exchange of the *u*-quark lines between the initial and final state. However, they are not treated as the signal diagrams here, because they contain the gluon, \(Z^0\) or photon propagator in the *t*- or *u*-channel and their contribution to the signal cross section is negligible anyway, which has been checked by direct computation.

The rest of the article is organized in the following way. The possible effect of the anomalous top-Higgs coupling on the unpolarized cross section of the process of \(t\bar{t}H\) production at the LHC are analyzed in Sect. 2, our results are presented in Sect. 3 and, finally, some concluding remarks are contained in Sect. 4.

## 2 Effects of the anomalous top-Higgs coupling

*f*and \(f'\) describe, respectively, the scalar and pseudoscalar departures from the purely scalar top-Higgs Yukawa coupling of SM, which is reproduced for \(f=1\) and \(f'=0\). The allowed regions of the \((f,f')\) plane, according to the analysis of Ref. [20] performed at the 68 and 95 % confidence level, are plotted in Fig. 1 of Ref. [21]. They are derived from the constraints on the

*Hgg*and \(H\gamma \gamma \) couplings from the Higgs boson production and its decay into \(\gamma \gamma \), which among others involve assumptions on the Higgs boson couplings to other fermions and bosons, and hence are model dependent. Therefore, we will not stick to them in the next section, where we will illustrate the effects of \(f'\) on the process of associated production of the top-quark pair and Higgs boson from which the direct constraints on

*f*and \(f'\) can be derived.

*h*is a scalar representing a product of the Higgs boson propagator carrying the four-momentum

*q*with the \(Hb\bar{b}\) vertex,

*u*(

*v*) is the Dirac spinor representing the off-shell

*t*-quark (\(\bar{t}\)-quark) of the four-momentum \(p_t\) (\(p_{\bar{t}}\)) that decays into the

*b*-quark (\(\bar{b}\)-quark) and off-shell \(W^+\) (\(W^-\)) boson, \(\varepsilon \) is a polarization four-vector representing the gluon propagator contracted with the \(u\bar{u} g\) vertex, \(g_s\) is the strong coupling constant and \(M=\sqrt{m_t^2-im_t\Gamma _t}\approx m_t-\frac{i}{2}\Gamma _t\) is a complex mass parameter that replaces the mass \(m_t\) in the top-quark propagator in order to regularize the pole arising if its denominator approaches zero. After some simple algebra Eqs. (5) and (6) can be written in the following form: Now, let us note that, as in the process of \(t\bar{t} H\) production in \(e^+e^-\) collisions that was considered in Refs. [16, 17, 18], the dominant contribution to the cross section comes from the phase space region, where both the

*t*-quark and the \(\bar{t}\)-quark are close to their mass shells and hence the off-shell spinors

*u*and

*v*should satisfy the following approximate equations: Using Eqs. (9) in (7) and (10) in (8), and neglecting terms \(\sim \Gamma _t\) in the numerators, we get the following approximate expressions for the amplitudes: and for a sum of the two:In order to calculate the sum over polarizations of the squared module of the matrix element \(\sum _\mathrm{pol.}\left| M_a\right| ^2\), we take into account the approximate completeness relations for the spinors

*u*and

*v*:and note that the off-shell polarization four-vectors \(\varepsilon \) are real, as they are defined in the following way:

*u*-quark in initial state, which are calculated according to Eqs. (5) and (6) of Ref. [27], are real if the momenta \(\vec {p}_1\) and \(\vec {p}_2\) are antiparallel. ThusMore simplified analytic form of Eq. (16) is irrelevant, as the calculation of the cross section will be performed numerically anyway, but let us note that only the terms on the r.h.s. of Eq. (16) that contain \(\gamma _5\) may be proportional to the product \(ff'\). However, if we use the relation Open image in new window in the second and third term and the relation Open image in new window in the second term, and then use the relationin the last term on the r.h.s. of Eq. (16), we see that the dependence on \(ff'\), and thus a sensitivity to the sign of either

*f*or \(f'\), disappears in the unpolarized cross section of the hard-scattering process \(u \bar{u} \;\rightarrow \; b u \bar{d} \bar{b} \mu ^{-} \bar{\nu }_{\mu } b \bar{b}\). Let us note that the same arguments can easily be repeated for the amplitudes of the Feynman diagrams of Fig. 1, which dominate the \(t\bar{t} H\) production through the gluon fusion process (2). We would like to stress here that all the above approximations are used for the sake of the argument in this section only and are not used to obtain the full results presented in Sect. 3.

## 3 Results

*i*and

*j*, respectively, \(s' = x_1 x_2 s\) is the reduced center of mass energy squared,

*Q*is the factorization scale and we take into account the following pairs of partons (

*i*,

*j*): (

*g*,

*g*), \((u,\bar{u})\), \((\bar{u},u)\), \((d,\bar{d})\), \((\bar{d},d)\) in the sum. We use MSTW LO parton distribution functions [29] at the factorization scale \(Q=\sqrt{m_t^2+\sum _jp_{Tj}^2}\), where \(p_{Tj}\) is the transverse momentum of the final state quark or antiquark of process (18). The calculation is performed separately for the gluon fusion (2) and each of the quark–antiquark hard-scattering processes (3). We use the same physical input parameters and cuts (3.2)–(3.7), with \(m_{bb}^\mathrm{cut}=20\) GeV in (3.7), as in Ref. [19], and three different combinations of the scalar and pseudoscalar couplings of Lagrangian (4): \((f,f')=(1,0),(1,1),(1,-1)\). The first combination corresponds to the SM and the other two are chosen, just for the sake of illustration, beyond the allowed 95 % CL regions of the \((f,f')\) plane which, as discussed in the first paragraph of Sect. 2, are model dependent anyway. The cross sections of the hard-scattering processes considered are added afterwards, if necessary.

The differential cross sections of process (18) at the proton–proton center of mass energy of 14 TeV are plotted in Figs. 3, 4, 5, 6, 7 and 8 as functions of the rapidity and different angular variables of the final state muon, being referred to as the lepton. In Figs. 3, 4, 5, 6, 7 and 8, the left panels show the signal cross sections, which are computed with the signal \(t\bar{t}H\) production diagrams of the hard-scattering processes (2) and (3), as described in the previous sections, and the right panels show the complete LO cross sections, which are computed with the complete set of the LO Feynman diagrams of each of the hard-scattering processes considered. In each of the figures, the SM cross section of process (18) is plotted with gray shaded boxes and the contribution of the gluon fusion to it with the dashed-dotted line and the cross sections in the presence of the anomalous pseudoscalar coupling \(f'=1\) (\(f'=-1\)) are plotted with the solid (dotted) line. Thus, the shaded area above the dashed-dotted line shows the contribution of the quark–antiquark hard-scattering processes to either the \(t\bar{t}H\) signal or complete SM cross section. The effects of the anomalous pseudoscalar coupling \(f'=\pm 1\) are quite sizable in the signal cross sections which become by about 50 % bigger than in the SM. If all the LO Feynman diagrams are taken into account the effects remain the same in absolute terms, but their relative size is substantially smaller, as the anomalous top-Higgs coupling (4) practically does not alter the off-resonance background contributions which substantially increase the cross section of process (18). The shape of each of the differential cross sections plotted in Figs. 3, 4, 5, 6, 7 and 8 is hardly changed in the presence of the anomalous coupling \(f'=\pm 1\). Moreover, the cross sections for \(f'=1\) and \(f'=-1\) look almost identical, which means that the process is practically insensitive to a sign of \(f'\), in accordance with the discussion of Sect. 2.

The individual contributions of the \(u\bar{u}\)- and \(\bar{u} u\) hard-scattering processes to the \(t\bar{t} H\) signal differential cross sections of process (18) at \(\sqrt{s}=14\) TeV are plotted in Figs. 9, 10 and 11, as functions of the lepton rapidity, cosine of the lepton angle with respect to the beam and cosine of the lepton angle with respect to the Higgs boson in the laboratory (LAB) frame, respectively. The relative effects of the anomalous pseudoscalar coupling \(f'\) in the plots of Figs. 9, 10 and 11 are approximately the same as in the full signal cross sections plotted in the right panels of Figs. 3, 4, and 8, respectively, and again there is practically no sensitivity to the sign of \(f'\). Taking into account the off-resonance background contributions to any of the quark–antiquark hard-scattering processes does not change this conclusion either, i.e., the shapes and relative effect of the anomalous coupling \(f'\) remain practically the same for all the distributions considered.

## 4 Conclusions

We have complemented the analysis of the influence of the anomalous Higgs boson coupling to the top quark on the secondary lepton distributions in the process of associated production of the top-quark pair and Higgs boson in the proton–proton collisions at the LHC of Ref. [19] by taking into account contributions of the quark–antiquark annihilation hard-scattering processes. Although the gluon fusion mechanism dominates the \(t\bar{t} H\) production through process (18) at \(\sqrt{s}=14\) TeV, the contribution of quark–antiquark hard-scattering processes (3) is quite substantial and, therefore, should be taken into account in the analyses of data. Moreover, we have explained why the effects of the scalar and pseudoscalar anomalous couplings in the unpolarized cross section of the process are completely insensitive to the sign of either of them.

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