# Vector-boson pair production and electroweak corrections in Open image in new window

## Abstract

The detailed study of vector-boson pair production processes at the LHC will lead to a better understanding of electroweak physics. As pointed out before, a consistent inclusion of higher-order electroweak effects in the analysis of corresponding experimental data may be crucial to properly predict the relevant phenomenological features of these important reactions. Those contributions lead to dramatic distortions of invariant-mass and angular distributions at high energies, but may also significantly affect the cross section near threshold, as is the case e.g. for Z-pairs. For this reason, we present an analysis of the next-to-leading-order electroweak corrections to WW, WZ, and ZZ production at the LHC, taking into account mass effects as well as leptonic decays. Hence, our predictions are valid in the whole kinematic reach of the LHC and, moreover, respect the spin correlations of the leptonic decay products at next-to-leading-order accuracy. Starting from these fixed-order results, a simple and straightforward method is motivated to combine the electroweak corrections with state-of-the-art Monte Carlo predictions, focusing on a meaningful combination of higher-order electroweak and QCD effects. To illustrate our approach, the electroweak corrections are implemented in the HERWIG++ generator, and their phenomenological effects within a QCD environment are studied explicitly.

## Keywords

Transverse Momentum Pair Production Parton Shower Electroweak Correction Large Transverse Momentum## 1 Introduction

Vector-boson pair-production processes play a central role in LHC phenomenology. These processes are not only of great importance with respect to background analyses in Standard-Model (SM) Higgs production, they will also provide deeper insight into the structure of the electroweak interaction at highest energies. This is particularly true for the future high-luminosity run of the LHC at a center-of-mass (CM) energy of 13 TeV, which will allow for an unprecedented accuracy in the analysis of vector-boson interactions at the TeV scale. Consequently, theoretical prediction with high accuracy is needed for this important class of processes.

Given the experimental accuracy already achieved by LHC experiments in the 7- and 8-TeV runs [1, 2, 3, 4, 5, 6], at least the next-to-leading-order (NLO) QCD corrections are mandatory for a robust prediction of \(V\)-boson pair-production processes (for selected references see Refs. [7, 8]). In addition, important steps toward NNLO predictions for massive vector-boson pair-production processes have been made [9, 10, 11]. (As far as photon-pair and Z\(\gamma \) production at the LHC are concerned, the full strong two-loop corrections are known even fully differentially [12, 13, 14]). In particular, approximate NNLO results for \(\mathrm {W^+Z}\) and WW production have been provided for high-transverse-momentum observables [15, 16], as well as for WW production in the threshold limit [17]. Recently, also the full NNLO corrections to the total Z-pair production cross section were computed [18], reducing the remaining theory uncertainties to a level of only 3 %.

Having reached this high level of accuracy in the QCD predictions, also electroweak (EW) corrections (and other related electroweak effects) are becoming more and more important, and a lot of activity has taken place also in this field. In particular, the interplay of EW corrections and anomalous couplings has been investigated in Ref. [19]. The corresponding EW corrections have been computed in Ref. [20] in the high-energy limit, including leptonic decays and off-shell effects. Recently, also the full EW corrections to W-pair production, also taking into account mass effects as well as off-shell effects, have been evaluated for the leptonic final state [21]. Leading two-loop effects at high transverse momenta were evaluated in Ref. [22] for W-pairs. A detailed analysis of on-shell \(V\)-boson pair production (\(V={\mathrm {W}}^\pm ,{\mathrm {Z}}\,\)) and \(\gamma \gamma \) production including EW corrections has been provided in Refs. [7, 8], consistently including all mass effects. Recently, a detailed review of NLO effects in pair production of massive bosons has been provided, emphasizing the importance of photon-induced contributions [23].

Expecting first results for the full NNLO QCD corrections to W-pair production in the near future [24], a natural next step would be the combination of EW and QCD predictions at \(\mathcal {O}(\alpha _s\alpha )\) accuracy on a consistent theory basis, as has been partially done for the Drell–Yan process [25, 26, 27, 28, 29, 30, 31, 32, 33] already, where important contributions from mixed EW\(\times \)QCD corrections in the resonance region were found [34]. However, these multiscale two-loop calculations are beyond feasibility at present. Nevertheless, at least a pragmatic prescription of combining QCD predictions with EW corrections is desirable, aiming for a combination of EW precision with standard Monte Carlo (MC) tools.

In this work we extend the above results in two ways. In Sect. 2, in addition to predictions for W-pair production, also a first study of EW corrections to \({\mathrm {W}}{\mathrm {Z}}\) and \({\mathrm {Z}}{\mathrm {Z}}\) production is presented, including mass effects as well as leptonic decays, to allow for a realistic event definition in the leptonic decay modes. We point out that our results are not restricted to the high-energy regime but are also valid at moderate energies of \(\sim \)200 GeV, where already corrections of \(\sim \)5–10 % may be observed. Applying these results we propose, in a second step, a straightforward and simple strategy for the implementation of EW corrections in any state-of-the-art MC generator (Sect. 4), relying on \(K\)-factors for unpolarized two-by-two scattering and the assumption of factorization of EW and QCD effects, as will be motivated in Sect. 3. Our method will be tested against an alternative implementation method especially tailored for the HERWIG++ [35, 36] MC generator. In Sect. 5 selected numerical results obtained within the HERWIG++ setup will be discussed.

## 2 Electroweak corrections

As stated in the introduction, the complete evaluation of the combined QCD and electroweak corrections to gauge-boson pair production of order \(\alpha \alpha _s\) is presently out of reach. As a first step we, therefore, consider a factorized ansatz, where the kinematics of events with additional QCD radiation is mapped to effective two-body collisions, described by effective (squared) partonic energies and energy transfers \(\hat{s}\) and \(\hat{t}\). We assume that the bulk of the QCD corrections arises from events with soft or collinear emission, where the factorized ansatz is expected to work well. The EW corrections are taken directly from the result of the one-loop calculation, evaluated at the same kinematical point. This approach is expected to fail for events with large transverse momenta of the gauge-boson pair recoiling against a jet with large transverse momentum. These events, however, are of lesser relevance for the study of gauge-boson dynamics and can be eliminated by suitable cuts, as discussed in Sect. 4. The motivation of this approach will be discussed in Sect. 3, and details of the implementation are given in Sect. 4.

In the present section we concentrate on the electroweak corrections and motivate that indeed the bulk of the electroweak corrections can be collected in a \(K\)-factor which is given as a function of \(\hat{s}\) and \(\hat{t}\) only (Sect. 2.1). Photonic corrections (which evidently lead to a more complicated kinematic situation) can be split off such that the corresponding modifications of the electroweak corrections are small. This aspect will be investigated in Sect. 2.2.

A second simplification is introduced by applying a correction factor which does not depend on the helicities of the gauge bosons. In Sect. 2.3 we argue that this approximation still preserves the proper angular distributions and correlations of the Z and W decay products and investigate the phenomenological implications of this approximation in detail. Finally, the corrections as derived for on-shell gauge-boson production are applied for the cases where W or Z are slightly off mass shell (in the case of Z bosons we also include the amplitude where fermion pairs are produced through the virtual photon). The quality of this approximation at lowest order will also be discussed in Sect. 2.3. First, however, let us briefly recall the most important phenomenological features of various EW effects in on-shell WW, WZ, and ZZ production at the LHC.

### 2.1 On-shell gauge-boson pair productions

Here, we summarize the combination of different electroweak effects in on-shell \(V\)-pair production which have been discussed in detail in Refs. [7, 8, 23]. For the numerical implementation, we use the default setup defined in Refs. [7, 8].

^{1}The situation is different for the WZ channel. In this case, the interplay between CKM angles and PDFs leads to a shift of the tree-level prediction of about one percent. For the radiative corrections the CKM matrix can, therefore, still be set to unity.

The above picture significantly changes if angular distributions of the W-pair are studied at high invariant masses. This can be seen in Fig. 1 (bottom) where distributions of the rapidity gap of the two Ws are shown for \(M_{\mathrm {WW}}>\) 1,000 GeV. While the genuine EW corrections drastically reduce the differential cross section at high \(p_{{\mathrm {T}},\mathrm {W}}\), corresponding to small rapidity gap, the photon-induced contributions significantly increase the rate at small scattering angles, corresponding to large rapidity gap. As a result, a dramatic distortion of the angular distribution is visible which might easily be misinterpreted as signal of anomalous couplings.

We point out that the photon-induced corrections presented above (which are obtained using the MRST2004qed PDF set [39] for the photon density) suffer from a large systematic error stemming from our ignorance of the photon content of the proton. This becomes obvious looking at Fig. 25 of Ref. [41], where the NNPDF2.3QED [41] set has been used to estimate the error on the \(\gamma \gamma \)-induced W-pair cross section. A relative error of \(\pm 50~\%\) on the leading-order (LO) cross section at \(M_{\mathrm {WW}} =\) 1,000 GeV can be deduced, solely induced by the photon PDF error. This picture indicates that a significant improvement in the determination of the photon PDFs is mandatory to reliably predict the W-pair production cross section at high energies.

### 2.2 \(K\)-factors for the electroweak corrections

Similar considerations apply to di-photon production, and results analogous to ZZ production are also shown in Fig. 4. Again the relative contribution from purely photonic corrections is small and the two-body approximation reproduces the full answer to better than 1 %. The correction factors \(K^{\gamma \gamma }_{\mathrm{u}{\bar{\mathrm{u}}}}\), \(K^{\gamma \gamma }_{\mathrm{d}{\bar{\mathrm{d}}}}\) and\( K^{\gamma \gamma }_{\mathrm{b}{\bar{\mathrm{b}}}}\) are defined in an obvious way. The results presented in Fig. 4 were obtained using the default setup as defined in Ref. [8].

The situation is more involved in the case of W-pair and WZ production where weak and electromagnetic corrections are intimately intertwined. As is well known, virtual photonic corrections are required to arrive at an ultraviolet finite answer. The resulting infrared divergencies are then canceled by real radiation, the remaining collinear singularities are finally absorbed into a redefinition of the PDFs. Since one is now dealing partially with a three-body final state, the direct use of a \(K\)-factor which depends on \(\hat{s}\) and \(\hat{t}\) only is nontrivial.

### 2.3 Gauge-boson polarization and four-lepton production

Our corrections are presented for unpolarized gauge bosons, which in the case of W and Z are observed through their decay products. The distributions of the decay products, however, are affected by the boson polarization. Hence an additional complication could result from the fact that the polarization pattern of the gauge bosons is modified by the radiative corrections. In principle one would have to employ \(K\)-factors for the full set of helicity amplitudes. However, as demonstrated in Ref. [8] for ZZ production, in practice a fairly simple pattern emerges. Let us first consider the case of Z pairs: For small transverse momenta the electroweak corrections are small (about \(-4~\%\)) and of similar magnitude for all four combinations of transverse and longitudinal polarizations. For large transverse momenta one single configuration dominates completely and corrections for the subdominant combinations are irrelevant. This feature has been demonstrated in Table 7 of Ref. [8], where the cross sections and the corrections are displayed in the low-, intermediate- and large-\(p_{\mathrm {T}}\) region, separated according to longitudinal and transverse polarizations.

From these considerations it becomes clear that in the case of Z-pair production a single partonic \(K\)-factor is sufficient for large as well as for small transverse momenta, and polarizations of the gauge bosons and, correspondingly, the correlations between the decay products as predicted in Born approximation are maintained even after inclusion of the electroweak corrections. The situation is slightly different for W-pair (and also WZ) production. Here, roughly 10 % of the LO cross section are given by longitudinally polarized Ws even at high transverse momenta, and the corresponding relative EW corrections are substantially different compared to the transversely polarized case (see Fig. 7 of Ref. [22]). However, the numerical effects from the longitudinal polarization on the radiative corrections are small, and it is still sufficient—as will be shown later—to apply unpolarized \(K\)-factors to reproduce the full corresponding EW corrections with sufficient accuracy.

The corrections evaluated in Refs. [7, 8] and encoded in our \(K\)-factors were obtained for on-shell Z or W bosons. Any realistic simulation of four-fermion production must, necessarily, include contributions from off-shell configurations. In the case of Z also diagrams with off-shell Z replaced by virtual photons would be required for a description away from the Z peak. However, for the experimental analysis of gauge boson production the invariant mass of the decay products (lepton pairs or jets) must be restricted to an interval around the nominal mass, say \(|M_{l\bar{l}}-M_{\mathrm {Z}}|<25\ \mathrm{GeV}\), to suppress the admixture of virtual photons and enhance close-to-mass-shell gauge bosons. In this case the neglect of virtual photons as implemented in HERWIG++ can be justified^{2}.

In our approach off-shell effects and non-resonant contributions are consistently accounted for in the LO predictions, while at NLO the NWA is applied to compute the relative corrections. This approximation is well motivated, since off-shell effects in the EW corrections only amount to \(\sim \)0.5 %, as demonstrated in Ref. [21] for W-pair production.

From these considerations it can be expected that the dominant weak corrections to four-lepton production at the LHC are well described by process dependent \(K\)-factors which can be taken from the unpolarized results for the corresponding \(2 \rightarrow 2\) production process. The validity of the approximations discussed above will now be studied in detail.

For the evaluation of hadronic cross sections we use the CT10NLO PDF set [44] in the LHAPDF framework [38], and the CKM dependence in the WZ production channels is included at leading order, while in the computation of EW corrections the CKM matrix is set to unity.

At leading order we present full results, including non-resonant and off-shell effects, as well as results in two different approximations. As far as the full LO cross sections are concerned, we have checked that the difference between a naive fixed width implementation and results obtained in the Complex-Mass Scheme (CMS) [45, 46] is at the per-mill level and hardly visible. All results presented here for the full LO cross sections therefore correspond to the naive fixed-width implementation.

In addition to the full results, we provide the results for \(V\)-boson pair production in the double-pole approximation (DPA) originally discussed in Ref. [20]. Here, the amplitudes for V-pair production and decays are evaluated on-shell, but the Breit–Wigner shape of the resonance is included in the evaluation of the squared matrix elements to account for the dominant off-shell effects. We apply the on-shell projection procedure proposed in Ref. [47] to construct proper on-shell momenta of the intermediate bosons from the four-particle phase space. Note that in addition to the physical cuts displayed above, we impose a technical cut, \(m_{4l} > M_{V_1}+M_{V_2}\), on the 4-lepton invariant mass since the on-shell projection suggested in Ref. [47] only gives sensible results above threshold.

In the left panels of Figs. 5, 6 and 7 we present LO results for various typical differential distributions for processes (2.11) at LHC13, resepctively. Besides the full results, the respective approximate results in NWA and DPA are also shown, always taken in leading order.

The right-hand-side panels of the respective plots show the relative deviations of the NWA (\(\Delta _{\mathrm {LO}}^{\mathrm {NWA}}\)) and DPA (\(\Delta _{\mathrm {LO}}^{\mathrm {DPA}}\)) from the full results. For all pair-production channels one observes that the NWA overshoots the full LO predictions at the level of 5 %, while the DPA results give a good approximation valid at the 2–3 % level. From the upper right plot of Fig. 5, it becomes obvious that both approximate predictions become crude near the Z-pair production threshold where off-shell effects apparently become more important.

Let us now turn to the EW corrections. As stated before, we compute the full EW corrections to the respective polarized vector-boson pair-production processes, and include the spin correlations in the decays to leptons, which are treated at leading order. The actual computation is carried out in the well-established FeynArts/FormCalc/LoopTools [48, 49, 50, 51, 52, 53] setup already used in Refs. [7, 8], and Madgraph [54] was useful for internal checks. We do not take into account the EW corrections to the leptonic decay processes for various reasons. On the one hand, the bulk of the EW corrections to Z and W decay are given by final-state photon radiation (FSR), which leads to significant distortions of the phase-space distributions of the leptonic decay products. These FSR corrections, however, are included in HERWIG++ [55] in the YFS framework [56] and will therefore not be considered here. On the other hand, electroweak corrections to the inclusive boson decay widths are implicitly included in the experimentally determined values for the branching ratios used in the HERWIG++ framework. Additionally, we strictly stick to the NWA for the computation of the EW corrections. In this simplified approach, the corrections completely factorize into corrections either to the production or the decay process. No non-factorizable corrections, connecting production and decay, have to be considered. Those contributions have to be taken into account using the DPA as demonstrated in Ref. [20]. However, it is well known that the non-factorizable corrections largely cancel in sufficiently inclusive observables [57].

In addition to the full EW corrections \(\delta _{\mathrm {EW}}^\mathrm {full}\) (which contain proper spin correlations and, in the case of WW and WZ production, also the full set of QED corrections to the respective production process) approximate results \(\delta _{\mathrm {EW}}^{\mathrm {V+E}}\), employing the virtual+endpoint (V+E) approximation, are presented in the same plots. In this case unpolarized on-shell \(K\)-factors have been used to obtain the relative corrections, as detailed in Sect. 2.2. One observes that the approximate ansatz gives an almost perfect approximation for the full result, in general better than 1 %. The best agreement is observed for ZZ production, while for WW production a slight discrepancy is visible. This can be understood recalling that photon radiation and related QED corrections are largest for WW production, as has been demonstrated in Ref. [8], while they remain small in the case of Z pairs. In general, the agreement between the full result and the V+E approximation is even better than expected. As a conclusion one finds that it is justified to use unpolarized \(K\)-factors in the V+E approximation to describe vector-boson pair production at the LHC at sufficient accuracy.

## 3 Electroweak and QCD corrections: combined

As stated in the introduction, the complete treatment of combined QCD and electroweak corrections, involving e.g. two-loop terms of order \(\alpha _s\alpha _\mathrm{weak}\) is presently out of reach. Consequently neither an additive treatment of the corrections, \((1+\delta _\mathrm{QCD}+\delta _\mathrm{weak})\), nor a multiplicative one, \((1+\delta _\mathrm{QCD})(1+\delta _\mathrm{weak})\), will lead to the correct result. However, the bulk of the QCD corrections for the processes under consideration is related to soft or collinear gluon radiation from the incoming quark–antiquark system. Soft radiation leaves the initial state practically unchanged, the quarks remain close to their mass shell and the weak corrections can be taken from the \(\hat{s}\) and \(\hat{t}\) dependent \(K\)-factor.

A similar line of reasoning is applicable to hard collinear radiation which leads to final states with vanishing or small transverse momentum of the diboson system. Let us assume that a collinear gluon is radiated from the incoming (anti-)quark, which subsequently initiates the boson pair production. Also in this case the (anti-)quark stays close to its mass shell. The scattering angle of the \(q_1\bar{q}_2\rightarrow V_1V_2\) reaction in the \(V_1V_2\) rest frame can again be directly identified with the scattering angle of the partonic reaction. A similar line of reasoning applies to reactions with quarks or antiquarks originating from gluon splitting.

Diboson events with large transverse momenta necessarily require the presence of at least one hard quark or gluon jet, and electroweak corrections would have to be evaluated separately for this class of processes. As long as they can be treated as a small admixture to the diboson sample, suppressed by an additional factor \(\alpha _s\), the distortion of the weak corrections should not lead to a significant error for the inclusive sample. If one is interested specifically in the analysis of the diboson process, a cut on the transverse momentum of the dibosons system will eliminate the pollution with events of a very different nature. Let us discuss this important issue in some more detail. As pointed out by several groups [7, 15], at large transverse momenta \(V\)-pair production is dominated by new topologies which are absent at lowest order in QCD. These topologies correspond to \(V\)+jet production with the radiation of an additional \(V\) from the quark jet rather than being a correction to \(V\)-pair production and spoil the perturbative series for the prediction of leptonic observables at high transverse momenta. They lead to huge QCD \(K\)-factors together with large residual scale uncertainties. To improve the corresponding theory predictions the authors of Ref. [15] have provided approximate NNLO QCD predictions for these particular observables in WZ production, applying the LoopSim method [58]. They observe pronounced shifts of the predictions going from NLO to NNLO and at the same time a significant reduction of the theory uncertainties. In this work, however, we follow another strategy to stabilize the problematic high-\(p_{\mathrm {T}}\) observables, employing suitable restrictions on the transverse momentum of the 4-lepton system, as will be detailed in Sect. 5.

In the present section a fairly general prescription has been suggested how to implement weak corrections into a generic Monte Carlo program which includes QCD corrections and hadronization already. Indeed this prescription allows for an *a posteriori* application of EW corrections to any QCD Monte Carlo, at least as long as the partonic origin (\({\mathrm{u}{\bar{\mathrm{u}}}}\) vs. \(\mathrm{d}{\bar{\mathrm{d}}}\)) of the final state remains under control. In the next section a slightly different approach will be described which is specifically tailored to the program HERWIG++. In this case a partonic \(\hat{s}\) and \(\hat{t}\) is introduced in the program from the very beginning and, in the limit of diboson events with small transverse momenta, coincides with the prescription described above. In the following section this correspondence will be investigated in more detail.

## 4 Implementation into Open image in new window

Our starting point of the implementation of the EW corrections in HERWIG++ is the electroweak \(K\)-factor. Following the strategy of multiplicative QCD and EW corrections we reweight the events that have been generated in HERWIG++ as the hard processes. For vector-boson pair production HERWIG++ delivers unweighted events. Hence we can compute \(K(\hat{s}, \hat{t})\) and use this directly as a reweighting factor for each event such that \(K(\hat{s}, \hat{t}) < 1\) leads to a suppression of events with given \((\hat{s}, \hat{t})\) while \(K(\hat{s}, \hat{t}) > 1\) leads to an enhancement. The actual implementation of a reweighting factor for a given hard event is straightforward in HERWIG++ and ThePEG once the variables \((\hat{s}, \hat{t})\) are known.

Let us discuss the kinematics of our events in more detail. For EW corrections to the Born process the calculation of a \(K\)-factor is straightforward as we can directly access the kinematic setup of the hard process once this is generated. In this case \((\hat{s}, \hat{t})\) can be computed uniquely. As soon as we want to apply the EW corrections to an event that is generated from an NLO QCD matrix element this is no longer the case. In this case we face the complication that an event with real radiation is not described by \(2\rightarrow 2\) kinematics anymore.

In the HERWIG++ implementation we find exactly this prescription. In a first step we generate an event with kinematical configuration \(\Phi _B\). Technically, this is already the hard process. Only in a second step, already as part of the parton shower algorithm, the potential hard emission with relative kinematics \(\Phi _R\) is generated according to the Sudakov form factor (4.3). Once this is done, the default parton shower is used as at this point, all terms will become formally higher than next-to-leading order and the default parton shower is computationally much simpler than the Sudakov form factor (4.3).

As the hard emission from POWHEG is technically already part of the parton shower, we have direct access to the Born-type variables \(\Phi _B\) in the hard subprocess and hence we may easily compute the kinematic variables \((\hat{s}, \hat{t})\) for every event. In effect, this assumes that the EW corrections are applied only on the level of Born-type kinematics and are not strongly influenced by the hard emission. In fact, by applying a suitable veto, we later also focus our analysis to regions where the transverse momenta generated by hard gluon emissions are not too large. This veto will suppress events where gauge-boson pairs are accompanied by additional hard quark or gluon jets, leaving the \(q\bar{q}\) events largely unaffected. This also enforces the kinematics to be reasonably close to a Born configuration in order to justify our approach.

In Fig. 8 we show histograms of the ratio \(\rho \) of vector and scalar sums of lepton transverse momenta that we finally apply the cut on. We show runs with and without NLO QCD corrections. We find that the chosen value \(\rho =0.3\) is a sensible choice for all three combinations of boson pairs. A good number of events is still available for the analysis while at the same time we find that the events with large distortions from hard radiation are vetoed with our selection. These are peaked at large values of the ratio in all three cases. In a full experimental analysis the value of \(\rho \) might be subject to optimization for the individual cases of vector-boson pairs.

In order to assess the sensitivity to the choice of partonic kinematic variables we have studied the impact of \(K(\hat{s}, \hat{t})\) with two additional choices for the kinematical variables for ZZ production, as in this case we have full access to the kinematics of the final state.

Let us call the variables from the direct access to the kinematics within HERWIG++ before the parton shower \((\hat{s}_\mathrm{hard}, \hat{t}_\mathrm{hard})\). As an alternative, we reconstruct the kinematics from the vector-boson final state as outlined in the previous section. Here, no knowledge of the initial-state partons is needed for the computation of the kinematic invariants. \(\hat{s}_\mathrm{rec}\) is given by the invariant mass of the vector-boson pair and \(\hat{t}_\mathrm{rec}\) is reconstructed from the scattering angle in the center-of-mass frame as proposed in (3.1)–(3.4). For illustration, we also consider a choice of variables that is very likely to be wrong. We take the initial-state partons after the termination of the parton shower. This parton pair will have a much larger invariant mass \(\hat{s}_\mathrm{PS}\) due to the parton showering. We then find the four momenta of the outgoing vector bosons and compute \(\hat{t}_\mathrm{PS}\) with respect to this initial state. This last choice will demonstrate the sensitivity to the parton shower emissions. For each event produced by HERWIG++ we construct three sets of kinematic variables \((\hat{s}_i, \hat{t}_i)\) with \(i\in \{\mathrm{hard}, \mathrm{rec}, \mathrm{PS}\}\). Then we compute the three different \(K\) factors \(K_i\) from these three sets of variables. Taking \(K_\mathrm{hard}\) as a reference we compute the ratio \(K_i/K_\mathrm{hard}\) for each event. If the reconstruction would be insensitive to the choice of kinematics this ratio ought to be unity all the time.

In strong contrast, the EW \(K\)-factors based on the kinematics reconstruction from the final state compared to the \(K\)-factor based on the variables of the hard process inside the event generator are very close. Their ratio is very strongly peaked around one, demonstrating that the two prescriptions lead to nearly identical results.

In the same Fig. 13 we compare the results from runs with and without NLO QCD corrections. In both cases we get very similar results for the EW \(K\)-factor. The additional hard gluon from the real-emission graph distorts the kinematics that was reconstructed in the leading-order case only slightly. As expected the QCD corrections lead to slightly bigger difference between the two reconstruction schemes.

We conclude that our computation of the EW correction is very robust against small variations of the kinematics as long as the variables are sensibly chosen and a sensible veto is applied. The reconstruction of kinematics from the final state alone, as proposed in the previous section, is a viable choice. In contrast, naively ignoring the parton shower in the reconstruction of kinematics will lead to significantly different results.

## 5 Open image in new window results

Before we discuss the phenomenology of EW corrections in the HERWIG++ framework in detail, we would like to stress again that the multiplicative approach combining EW and QCD corrections introduced in this paper essentially requires a “back-to-back” signature of the vector bosons in the final state. Otherwise, events at high transverse momenta are dominated by hard QCD radiation, and the center-of-mass frame of the two vector bosons is strongly boosted in the transverse direction. In this kinematic regime, however, a naive factorization of EW and QCD corrections will almost surely fail, and substantial uncertainties due to missing terms of \(\mathcal {O}(\alpha \alpha _s)\) (and also \(\mathcal {O}(\alpha _s^2)\)) will arise. Therefore, we strongly recommend the implementation of the veto (4.4) (or any equivalent prescription) for the application of the \(K\)-factor approach described in this work.^{3}

Having established the role of the veto on the leptonic final state, we present results of differential distributions in leptonic observables. We apply the same selection of final states as described above in Sects. 2.3 and 4. Now, the leptons are, however, selected from a full hadronic final state with an additional isolation cut of \(R=0.2\). Furthermore, the final state is of course modified by parton showers and hadronization as well as additional soft and collinear photon radiation. We left the underlying event switched off as we expect only a small effect for the observables presented here. In all cases we have generated \(10\)M unvetoed events. The leptonic veto has only been applied at the analysis level.

In Fig. 14 we show a number of observables for the final state of \(\mathrm {ZZ}\) production. In all cases we show four lines: the leading-order result (LO), results with only electroweak (NLO EW) or QCD corrections (NLO QCD) applied and, finally, the result with the combined EW and QCD corrections in the multiplicative scheme as outlined above. In both cases, with and without NLO QCD corrections, the additional EW correction is as sizable as in the partonic case, i.e. of the order of \(-5\,\%\) for small \(m_{4l}\), reaching up to \(-20\,\%\) for \(m_{4l}\) close to 1 TeV or \(p_{{\mathrm {T}},l\bar{l}}\) close to 500 GeV. The rapidity distributions, shown in the lower two plots of Fig. 14, receive the correction of \(-4~\%\) typical for the low-\(\hat{s}\) configuration.

A similar picture emerges in the case of WZ production which we show in Fig. 15 for \(\sqrt{s}=13\,\)TeV. Here, the EW corrections are smaller than in the ZZ case. In every observable we find that the EW corrections act quite similar on the final states with and without NLO QCD corrections. While the QCD corrections are moderate, at the level of 20 %, the EW corrections vary between zero and \(-20\,\%\) and are again sizable for high transverse momenta of the Z bosons.

Finally, in Fig. 16 we consider selected observables for the case of W-pair production at 13 TeV. Here, the EW corrections are slightly larger than in the WZ case, but the overall picture remains the same. The QCD corrections are quite large but tamed by our veto on the leptonic final state, typically of the order of 20 %. The EW corrections are typically of the order of 5 % but again sizable in the case of large lepton transverse momentum, where they can completely compensate the QCD corrections.

## 6 Summary and conclusions

We have computed the full NLO EW corrections to resonant vector-boson pair production at the LHC, taking into account leptonic decays and corresponding spin correlations. We propose a simple and straightforward method—relying on unpolarized \(2\rightarrow 2\) \(K\)-factors—to implement our results in any state-of-the-art MC generator.

The EW corrections are combined with precise QCD predictions in a multiplicative approach, which is assumed to provide reliable results in a leading-order-like kinematic regime. We enforce this by application of a kinematic veto based on the transverse momenta of the leptonic decay products. To estimate the effect of the veto on QCD uncertainties from missing higher orders, we vary the renormalization and factorization scale. A similar behavior is observed for inclusive and exclusive cross sections, suggesting uncertainties of the order of 10–20 %. The crossing of the error bands for \(p_{{\mathrm {T}},l\bar{l}}\) around 120 GeV, as observed in Fig. 12, should not be interpreted as vanishing theory uncertainty. It will be affected by a NNLO calculation and deserves further studies.

We emphasize that our method also allows for an *a posteriori* implementation of EW \(K\)-factors into MC samples that have already been generated. To demonstrate the practicability of our approach, we have included our corrections in the HERWIG++ MC generator and presented various distributions for four-lepton production at the LHC obtained in the HERWIG++ setup, including EW corrections, NLO QCD corrections matched to parton showers, as well as hadronization effects. In the future our method could also be applied to other process classes, such as \(V\)+jet production at the LHC, allowing for phenomenological studies that combine EW precision on the one hand and an adequate treatment of dominating QCD effects on the other.

## Footnotes

- 1.
We point out that a non-vanishing top-quark mass is consistently included in the computation of the one-loop contributions discussed in this paper.

- 2.
The HERWIG++ implementation of \(V\)-pair production [43] relies on the double-pole approximation, where only doubly resonant contributions are taken into account including off-shell effects.

- 3.
Furthermore, a “back-to-back” requirement for the final-state vector bosons will also reduce the admixture of massive-vector-boson radiation and \(V_1V_2\gamma \) events, as well as contributions from quark–photon-induced processes, which suffer substantially from the large photon-PDF error quoted by the NNPDF collaboration.

## Notes

### Acknowledgments

This work was supported by the DFG Sonderforschungsbereich/Transregio 9 “Computergestützte Theoretische Teilchenphysik”. SG acknowledges support from the EU Initial Training Network “MCnetITN” and the Helmholtz Alliance “Physics at the Terascale”.

## References

- 1.G. Aad et al. [ATLAS Collaboration], JHEP
**1303**, 128 (2013). arXiv:1211.6096 [hep-ex] - 2.G. Aad et al. [ATLAS Collaboration], Phys. Rev. D
**87**, 112001 (2013). arXiv:1210.2979 [hep-ex] - 3.G. Aad et al. [ATLAS Collaboration], Eur. Phys. J. C
**72**, 2173 (2012). arXiv:1208.1390 [hep-ex] - 4.S. Chatrchyan et al. [CMS Collaboration]. arXiv:1306.1126 [hep-ex]
- 5.S. Chatrchyan et al. [CMS Collaboration], Phys. Lett. B
**721**, 190 (2013). arXiv:1301.4698 [hep-ex] - 6.S. Chatrchyan et al. [CMS Collaboration], JHEP
**1301**, 063 (2013). arXiv:1211.4890 [hep-ex] - 7.A. Bierweiler, T. Kasprzik, H. Kühn, S. Uccirati, JHEP
**1211**, 093 (2012). arXiv:1208.3147 [hep-ph] - 8.A. Bierweiler, T. Kasprzik, J.H. Kühn. arXiv:1305.5402 [hep-ph]
- 9.F. Caola, J.M. Henn, K. Melnikov, V.A. Smirnov. arXiv:1404.5590 [hep-ph]
- 10.T. Gehrmann, L. Tancredi, E. Weihs, JHEP
**1308**, 070 (2013). arXiv:1306.6344 [hep-ph] - 11.G. Chachamis, M. Czakon, D. Eiras, JHEP
**0812**, 003 (2008). arXiv:0802.4028 [hep-ph] - 12.Z. Bern, A. De Freitas, L.J. Dixon, JHEP
**0109**, 037 (2001). hep-ph/0109078 - 13.S. Catani, L. Cieri, D. de Florian, G. Ferrera, M. Grazzini, Phys. Rev. Lett.
**108**, 072001 (2012). arXiv:1110.2375 [hep-ph] - 14.M. Grazzini, S. Kallweit, D. Rathlev, A. Torre. arXiv:1309.7000 [hep-ph]
- 15.F. Campanario, S. Sapeta, Phys. Lett. B
**718**, 100 (2012). arXiv:1209.4595 [hep-ph] - 16.F. Campanario, M. Rauch, S. Sapeta. arXiv:1309.7293 [hep-ph]
- 17.S. Dawson, I.M. Lewis, M. Zeng. arXiv:1307.3249 [hep-ph]
- 18.F. Cascioli, T. Gehrmann, M. Grazzini, S. Kallweit, P. Maierhfer, A. von Manteuffel, S. Pozzorini, D. Rathlev et al. arXiv:1405.2219 [hep-ph]
- 19.E. Accomando, A. Kaiser, Phys. Rev. D
**73**, 093006 (2006). hep-ph/0511088 - 20.E. Accomando, A. Denner, A. Kaiser, Nucl. Phys. B
**706**, 325 (2005). hep-ph/0409247Google Scholar - 21.M. Billoni, S. Dittmaier, B. Jäger, C. Speckner. arXiv:1310.1564 [hep-ph]
- 22.J.H. Kühn, F. Metzler, A.A. Penin, S. Uccirati, JHEP
**1106**, 143 (2011). arXiv:1101.2563 [hep-ph] - 23.J. Baglio, L.D. Ninh, M.M. Weber. arXiv:1307.4331 [hep-ph]
- 24.G. Chachamis. arXiv:1312.4220 [hep-ph]
- 25.R. Boughezal, Y. Li, F. Petriello. arXiv:1312.3972 [hep-ph]
- 26.W.B. Kilgore, C. Sturm. arXiv:1107.4798 [hep-ph]
- 27.A. Kotikov, J.H. Kühn, O. Veretin, Nucl. Phys.
**B788**, 47–62 (2008). hep-ph/0703013 [HEP-PH]Google Scholar - 28.Q.H. Cao, C.P. Yuan, Phys. Rev. Lett.
**93**, 042001 (2004). hep-ph/0401026 - 29.B.F.L. Ward, C. Glosser, S. Jadach, S.A. Yost, Int. J. Mod. Phys. A
**20**, 3735 (2005). hep-ph/0411047Google Scholar - 30.B.F.L. Ward, S.A. Yost, Acta Phys. Polon. B
**38**, 2395 (2007). arXiv:0704.0294 [hep-ph] - 31.A. Vicini et al., PoS RADCOR2007 (2007) 013Google Scholar
- 32.G. Balossini, G. Montagna, C.M. Carloni Calame, M. Moretti, O. Nicrosini, F. Piccinini, M. Treccani, A. Vicini, JHEP
**1001**(2010) 013. arXiv:0907.0276 [hep-ph] - 33.G. Balossini et al., Nuovo Cim.
**123B**, 741 (2008)ADSGoogle Scholar - 34.S. Dittmaier, A. Huss, C. Schwinn. arXiv:1405.6897 [hep-ph]
- 35.M. Bähr, S. Gieseke, M.A. Gigg, D. Grellscheid, K. Hamilton, O. Latunde-Dada, S. Plätzer, P. Richardson et al., Eur. Phys. J. C
**58**, 639 (2008). arXiv:0803.0883 [hep-ph] - 36.K. Arnold, L. d’Errico, S. Gieseke, D. Grellscheid, K. Hamilton, A. Papaefstathiou, S. Plätzer, P. Richardson et al. arXiv:1205.4902 [hep-ph]
- 37.A.D. Martin et al., Eur. Phys. J.
**C63**, 189–285 (2009). arXiv:0901.0002 [hep-ph] - 38.M.R. Whalley, D. Bourilkov, R.C. Group, in HERA and the LHC, ed. by A. de Roeck, H. Jung (CERN-2005-014, Geneva, 2005), p. 575. hep-ph/0508110
- 39.A.D. Martin, R.G. Roberts, W.J. Stirling, R.S. Thorne, Eur. Phys. J.
**C39**, 155–161 (2005). hep-ph/0411040Google Scholar - 40.M. Roth, S. Weinzierl, Phys. Lett. B
**590**, 190 (2004). hep-ph/0403200 - 41.R.D. Ball et al. [The NNPDF Collaboration]. arXiv:1308.0598 [hep-ph]
- 42.S. Dittmaier, Nucl. Phys. B
**565**, 69 (2000). hep-ph/9904440Google Scholar - 43.K. Hamilton, JHEP
**1101**, 009 (2011). arXiv:1009.5391 [hep-ph] - 44.H.-L. Lai, M. Guzzi, J. Huston, Z. Li, P.M. Nadolsky, J. Pumplin, C.-P. Yuan, Phys. Rev. D
**82**, 074024 (2010). arXiv:1007.2241 [hep-ph] - 45.A. Denner, S. Dittmaier, M. Roth, L.H. Wieders, Nucl. Phys. B
**724**, 247 (2005). hep-ph/0505042Google Scholar - 46.A. Denner, S. Dittmaier, Nucl. Phys. Proc. Suppl.
**160**, 22 (2006). hep-ph/0605312Google Scholar - 47.A. Denner, S. Dittmaier, M. Roth, D. Wackeroth, Nucl. Phys. B
**587**, 67 (2000). hep-ph/0006307Google Scholar - 48.J. Küblbeck, M. Böhm, A. Denner, Comput. Phys. Commun.
**60**, 165 (1990) Google Scholar - 49.H. Eck, J. Küblbeck, Guide to FeynArts 1.0, University of Würzburg (1992)Google Scholar
- 50.T. Hahn, Comput. Phys. Commun.
**140**, 418 (2001). hep-ph/0012260 - 51.T. Hahn, M. Pérez-Victoria, Comput. Phys. Commun.
**118**, 153 (1999). hep-ph/9807565Google Scholar - 52.T. Hahn, C. Schappacher, Comput. Phys. Commun.
**143**, 54–68 (2002). hep-ph/0105349Google Scholar - 53.G.J. van Oldenborgh, J.A.M. Vermaseren, Z. Phys.
**C46**, 425–438 (1990)Google Scholar - 54.J. Alwall et al., JHEP
**0709**, 028 (2007). arXiv:0706.2334 [hep-ph] - 55.K. Hamilton, P. Richardson, JHEP
**0607**, 010 (2006). hep-ph/0603034 - 56.D.R. Yennie, S.C. Frautschi, H. Suura, Ann. Phys.
**13**, 379 (1961)CrossRefADSGoogle Scholar - 57.P. Falgari, A.S. Papanastasiou, A. Signer, JHEP
**1305**, 156 (2013). arXiv:1303.5299 [hep-ph] - 58.M. Rubin, G.P. Salam, S. Sapeta, JHEP
**1009**, 084 (2010). arXiv:1006.2144 [hep-ph] - 59.S. Frixione, P. Nason, C. Oleari, JHEP
**0711**, 070 (2007). arXiv:0709.2092 [hep-ph] - 60.A. Buckley, J. Butterworth, S. Gieseke, D. Grellscheid, S. Höche, H. Hoeth, F. Krauss, L. Lönnblad et al., Phys. Rept.
**504**, 145 (2011). arXiv:1101.2599 [hep-ph] - 61.S. Gieseke, Prog. Part. Nucl. Phys.
**72**, 155 (2013)CrossRefADSGoogle Scholar

## Copyright information

**Open Access**This article is distributed under the terms of the Creative Commons Attribution License which permits any use, distribution, and reproduction in any medium, provided the original author(s) and the source are credited.

Funded by SCOAP^{3} / License Version CC BY 4.0.