Direct determination of sin 2 ϑ l eff at hadron colliders

We discuss the renormalization of the electroweak Standard Model at one loop using the leptonic effective weak mixing angle as one of the input parameters. We evaluate the impact of this choice in the prediction of the forward-backward asymmetry for the neutral current Drell-Yan process. The proposed input scheme is suitable for a direct determination of the effective leptonic weak mixing angle from the experimental data.


I. INTRODUCTION
The weak mixing angle [1][2][3][4] is a fundamental parameter of the theory of the electroweak (EW) interaction, as it determines the combination of the gauge fields associated to the third component of the weak isospin and to the hypercharge, yielding the photon and the Z boson fields. The leptonic effective weak mixing angle sin 2 ϑ l eff , defined at the Z resonance, has been proposed [5][6][7][8][9][10] as a quantity sensitive to new physics, offering the opportunity of a stringent test of the Standard Model (SM). The measurement at LEP/SLD [11,12] was later challenged by the CDF and D0 determinations [13] at the Fermilab Tevatron and more recently by the results from the LHC collaborations ATLAS [14], CMS [15], and LHCb [16]. Two conceptually different strategies can (and should) be pursued for the direct determination of sin 2 ϑ l eff : with, whenever possible, a model independent as well as a pure SM approach. The latter will be useful as an internal self-consistency check of the SM, through the comparison of the direct determination with the most precise available calculations of sin 2 ϑ l eff . In this paper we discuss the renormalization of the EW SM at one-loop level, using sin 2 ϑ l eff , as defined at LEP/SLD, as one of the input parameters in the EW gauge sector. Any simulation code implementing such a scheme will be able to provide theoretical templates for a direct sensible comparison with the experimental data, with the leptonic effective weak mixing angle used as a fit parameter and consistently treated in the evaluation of next-to-leadingorder (NLO) and higher-order corrections. The use of sin 2 ϑ l eff as input parameter of the electroweak sector has also been proposed in Refs. [17][18][19][20][21] in the framework of the high-precision measurements at the Z boson resonance and higher energies at future e þ e − colliders.

II. INPUT SCHEMES AND RENORMALIZATION
The choice of an input scheme in the EW gauge sector of the SM is relevant for two distinct reasons: (i) In a theoretical perspective, the prediction of an observable should be affected by the smallest possible parametric uncertainty. This goal can be achieved by using the best known measured constants, like, for instance, the fine structure constant α, the Fermi constant G μ , and the Z boson mass M Z . Furthermore, the convergence of the perturbative expansion used to predict an observable is an additional criterium to judge whether the chosen inputs describe the process already in lowest order with good accuracy and reabsorb in their definition large radiative corrections. This is the case, for instance, of the scheme which uses G μ , M Z , and the W boson mass M W , to describe processes at the electroweak and higher scales. (ii) The determination of a fundamental constant at high-energy colliders can be achieved through the comparison of kinematical distributions computed in a theoretical model, the so-called templates, with the experimental data. The fundamental constant must be a free parameter of the model and is varied in the fitting procedure. Only the input parameters of the model can be unambiguously determined, because they are the only ones which can be freely varied without spoiling the accuracy of the calculation, while any other quantity is a prediction expressed in terms of them. Typical examples have been M Z at LEP1 and M W at LEP2, Tevatron, and LHC. Following the second perspective, we discuss in this paper the formulation of a renormalization scheme which includes the leptonic effective weak mixing angle sin 2 ϑ l eff [5] as one of the input parameters. Such a scheme will allow us to exploit the Tevatron and LHC (and in particular the future HL-LHC) potential to provide very high precision measurements of the neutral channel (NC) Drell-Yan (DY) process and, in turn, of sin 2 ϑ l eff .

A. Input scheme definitions
A set of three commonly adopted SM Lagrangian input parameters in the gauge sector is e; M W ; M Z ; they have to be expressed in terms of three measured quantities, whose choice defines a renormalization scheme. The relation between e; M W ; M Z and the reference measured quantities has to be evaluated at the same perturbative order of the scattering amplitude calculation at hand and allows us to fix the renormalization conditions. The usual sets of reference measured quantities are α; M W ; M Z , which defines the onshell scheme; αðM Z Þ; M W ; M Z , which is a variant of the on-shell scheme and reabsorbs the large logarithmic contributions due to the running of the electromagnetic coupling from the scale 0 to M Z [22]; G μ , M W , M Z , which defines the G μ scheme and is particularly suited to describe DY processes at hadron colliders because it allows one to include a large part of the radiative corrections in the LO predictions, guaranteeing a good convergence of the perturbative series. For a detailed description of these schemes see Ref. [26]. The presence of M W among the input parameters is a nice feature in view of a direct M W determination at hadron colliders via a template fit method, as described above. On the other hand, these schemes are not suited for high-precision predictions, because of the "large" parametric uncertainties stemming from the present experimental precision on the knowledge of M W . In fact, for NC DY precise predictions, a LEP style scheme with α; G μ ; M Z would be preferred. However, in view of a direct SM determination of the quantity sin 2 ϑ l eff , also this scheme has its own shortcomings, because sin 2 ϑ l eff is a calculated quantity and cannot be treated as a fit parameter. With the aim of a direct sin 2 ϑ l eff SM determination, we discuss an alternative scheme, which includes the weak mixing angle as a SM Lagrangian input parameter, sin 2 ϑ, together with e and M Z . The experimental reference data are the Z boson mass value measured at LEP, the fine structure constant α, and sin 2 ϑ l eff as defined at LEP at the Z resonance. An additional possibility discussed in the following is to replace α with G μ . We will refer to these two choices as the ðα; M Z ; sin 2 ϑ l eff Þ and the ðG μ ; sin 2 ϑ l eff ; M Z Þ input schemes. At tree level sin 2 ϑ ¼ sin 2 ϑ l eff . The quantity sin 2 ϑ l eff is defined in terms of the vector and axial-vector couplings of the Z boson to leptons g l V;A , measured at the Z boson peak, or alternatively the chiral electroweak couplings g l L;R and reads (at tree level) [27] is the third component of the weak isospin and Q l is the electric charge of the lepton in units of the positron charge.

B. Renormalization
We implement the one-loop renormalization of the three input parameters by splitting the bare ones into renormalized parameters and counterterms where the bare parameters are denoted with subscript 0. The counterterms δM 2 Z and δZ e are defined as in the usual on-shell scheme. Complete expressions are given in Eqs. (3.19) and (3.32) of Ref. [28]. The counterterm δ sin 2 ϑ l eff is defined by imposing that the tree-level relation equation (1) holds to all orders. Considering the Zl þ l − vertex and neglecting the masses of the lepton l, the couplings g l L;R are replaced by the form factors G l L;R ðq 2 Þ [9] once radiative corrections are accounted for. The effective weak mixing angle has been defined at LEP/SLD by taking the form factors at q 2 ¼ M 2 Z : The form factors G l i can be computed in the SM in any input scheme that does not contain sin 2 ϑ l eff as input parameter, yielding in turn, via Eq. (6), a prediction for sin 2 ϑ l eff , as discussed at length in Refs. [29,30]. In this paper instead we consider the weak mixing angle as an input parameter. In order to fix its renormalization condition, we write Eq. (6) at one loop, where δg l L;R represent the effect of radiative corrections, expressed in terms of renormalized quantities and related counterterms, including δ sin 2 ϑ l eff . We do not consider NLO QED corrections because they factorize on form factors and therefore do not affect the sin 2 ϑ l eff definition. The effective weak mixing angle is defined to all orders by the request that the measured value coincides with the treelevel expression. The counterterm δ sin 2 ϑ l eff is fixed by imposing that the one-loop corrections to Eq. (1) vanish, namely, We remark that at one loop the condition in Eq. (8) holds also if sin 2 ϑ l eff is defined from the ratio of the real parts of G V and G A . Moreover, Eq. (8) remains unchanged if the complex-mass scheme [31][32][33] is used for the treatment of unstable particles. In fact, M Z becomes complex but sin 2 ϑ l eff and, consequently, g l L and g l R remain real. Therefore Eq. (8) is valid also in the complex-mass scheme without modifications.
From the OðαÞ corrections to the vertex Zl þ l − we obtain where δZ AZ contains the fermionic and bosonic contributions to the γZ self-energy corrections, while the second line of Eq. (9) stems from the vertex corrections and counterterm contributions. We remark that the γZ selfenergy does not contain enhanced terms proportional to m 2 t . The bosonic contributions in Eq. (9) form a gauge invariant set because they are a linear combination of the corrections to the left-and right-handed components of the Z decay amplitude into a lepton pair. The expressions of δZ AZ and δZ l L=R are given in Eqs. (3.19) and (3.20) of Ref. [28], respectively. If the complex-mass scheme is used, the expression of δZ AZ can be found in Eqs. (4.7) and (4.30) of Ref. [32]. In δZ l L=R we suppressed the lepton family indices. The vertex corrections δV L=R are given by 2) of Ref. [28], respectively. The renormalization condition that the measured effective leptonic weak mixing angle matches the tree-level expression to all orders in perturbation theory applies, following the LEP definition, to the real part of the ratio of the vector and axial-vector form factors. The latter develop, order by order, an imaginary part which is computed in terms of the input parameters and contributes to the scattering amplitude.

C. The G μ scheme
The muon decay amplitude allows to establish a relation between α, G μ , M Z , and sin 2 ϑ l eff which reads with the following expression for Δr, where s W ¼ sin ϑ l eff and c W ¼ cos ϑ l eff , respectively. We note the appearance of the combination ΔαðsÞ − Δρ, which differs from the corresponding one for Δr in the ðα; M W M Z Þ on-shell scheme ΔαðsÞ − where Σ AA T ðsÞ, Σ AZ T ðsÞ, Σ ZZ T ðsÞ, and Σ W T ðsÞ can be found in Eqs. (B.1)-(B.4) of Ref. [28].
Using Eq. (11) to derive an effective electromagnetic coupling, it is possible to convert results computed in the (α, M Z , sin 2 ϑ l eff ) scheme to the corresponding ones in the (G μ , sin 2 ϑ l eff , M Z ) scheme. The Δρ term present at OðαÞ in Eq. (11) accounts for one-loop quantum corrections growing like m t 2 . For convenience we can introduce the quantity , which represents the m 2 t dependent part of Δρ defined in Eq. (15). This can be resummed to all orders, together with the irreducible two-loop contributions Δρ ð2Þ , computed in the heavy top limit in Ref. [34]. In the following predictions for the (G μ , sin 2 ϑ l eff , M Z ) scheme, we include the effect of the universal m t 2 corrections at two loops with the replacement G μ → G μ ð1 þ Δρ ð1Þ þ Δρ ð2Þ Þ after subtracting the Δρ ð1Þ contributions already included in the one-loop calculation.

III. THE DRELL-YAN PROCESS
We study at NLO EW the NC DY process, in the setup described in [35] but without acceptance cuts on the lepton transverse momentum and pseudorapidity, with The distributions are simulated with the POWHEG code (Z_BMNNPV processes svn revision 3652, under the POWHEG BOX v2 framework) [36], focusing on the lepton-pair invariant mass forward-backward asymmetry The size of NLO and higher-order radiative corrections, smaller than in the (G μ , M W , M Z ) case, can be ascribed to the choice as input parameters of the quantities that parametrize the Z resonance in terms of normalization (G μ ), position (M Z ) and shape (sin 2 ϑ l eff ), the latter two being defined at the Z resonance and thus reabsorbing a good fraction of the quantum corrections.
One of the main sources of parametric uncertainties is given, in any scheme with G μ as input, by the value of m t . In Fig. 3 we show the absolute variation of ΔA FB with respect to a change of AE1 GeV of m t around its central value, taken at m t ¼ 173.5 GeV, using the NLO accuracy with higher-order effects included, evaluated in the (G μ , sin 2 ϑ l eff , M Z ) (red lines) and (G μ , M W , M Z ) (blue lines) schemes. In the (G μ , sin 2 ϑ l eff , M Z ) scheme, the effect is well below the 2 × 10 −5 scale for A FB in the [60, 120] GeV mass range, almost vanishing in the Z peak region, while in the (G μ , M W , M Z ) case a variation of m t by AE1 GeV induces a shift ΔA FB of order 2 × 10 −4 . The very small dependence of A FB on the m t value is due to the cancellation of the overall normalization factor of the squared matrix element, between numerator and denominator of A FB , where the factor with the m t 2 dependence is present. Radiative corrections, logarithmic in m t , are by construction small at the Z peak, so that also the residual m t dependence is milder than in other invariant mass regions. In the (G μ , M W , M Z ) case instead the m t 2 dependence enters via the corrections to M W and affects the precise value of the on-shell weak mixing angle and, in turn, the shape of the A FB distribution.
In conclusion, we have presented an EW scheme that has sin 2 ϑ l eff , with exactly the same definition adopted at LEP/SLD, among the input parameters of the gauge sector and discussed its one-loop renormalization. In such a scheme the predictions of the NC DY process exhibit a faster convergence of the perturbative expansion and smaller m t parametric uncertainties, with respect to the (G μ , M W , M Z ) scheme. The presence of sin 2 ϑ l eff among the inputs allows its direct determination at hadron colliders and a closure test with a comparison against its best theoretical prediction in the SM based on the ðα; G μ ; M Z Þ input scheme. Such a scheme will allow the preparation of templates and the quantitative evaluation of the impact of radiative corrections and other theoretical uncertainties, in analogy with the study presented in Ref. [37] in the M W case. We implemented the scheme in the Z_BMNNPV svn revision 3652 processes under the POWHEG BOX v2 framework, but it can be easily implemented in any other code. FIG. 3. The absolute deviation between predictions on the lepton pair A FB as a function of M μ þ μ − , in the renormalization scheme with G μ , sin 2 ϑ l eff as input, with a variation of m t of AE1 GeV around the value m t ¼ 173.5 GeV. The precision of the calculation is NLO.