Global and optimal probes for the top-quark effective field theory at future lepton colliders

We study the sensitivity to physics beyond the standard model of precise top-quark pair production measurements at future lepton colliders. A global effective-field-theory approach is employed, including all dimension-six operators of the Warsaw basis which involve a top-quark and give rise to tree-level amplitudes that interfere with standard-model $e^+e^-\to t\,\bar t\to bW^+\bar bW^-$ ones in the limit of vanishing $b$-quark mass. Four-fermion and CP-violating contributions are taken into account. Circular-collider-, ILC- and CLIC-like benchmark run scenarios are examined. We compare the constraining power of various observables to a set of statistically optimal ones which maximally exploit the information contained in the fully differential $bW^+\bar bW^-$ distribution. The enhanced sensitivity gained on the linear contributions of dimension-six operators leads to bounds that are insensitive to quadratic ones. Even with statistically optimal observables, two centre-of-mass energies are required for constraining simultaneously two- and four-fermion operators. The impact of the centre-of-mass energy lever arm is discussed, that of beam polarization as well. A realistic estimate of the precision that can be achieved in ILC- and CLIC-like operating scenarios yields individual limits on the electroweak couplings of the top quark that are one to three orders of magnitude better than constraints set with Tevatron and LHC run I data, and three to two hundred times better than the most optimistic projections made for the high-luminosity phase of the LHC. Clean global constraints can moreover be obtained at lepton colliders, robustly covering the multidimensional effective-field-theory space with minimal model dependence.


Introduction
The particle content of the standard model (SM) is experimentally confirmed through the discovery of a state with properties compatible with that of its Higgs boson. Searches at the LHC exploring the TeV scale for signs of new physics have so far come up empty-handed. A complementary probe for physics beyond the standard model (BSM) is found in a precise characterization of standard-model processes with a pronounced BSM sensitivity. Using a global effective field theory, we evaluate in this paper the potential of future electronpositron colliders to constrain new physics affecting top-quark interactions.
The electroweak couplings of the top quark constitute one of the least precisely constrained quantities in the standard model. At the Tevatron and LHC, the electroweak qq → Z * /γ * → tt process is inaccessible. The hadron-collider experiments can probe the charged-current electroweak interactions of the top quark in its decay and single production. They have also started to probe the couplings of the top quark to the photon and Z boson in associated production.
Lepton colliders can probe top-quark couplings with neutral electroweak gauge bosons directly in the e + e − → tt pair production process. ILC studies [1,2] relying on a full simulation of the detector response and on estimates for the main systematic uncertainties have shown that cross section and forward-backward asymmetry measurements would yield percent-level determinations of the anomalous couplings of the top quark to the photon and Z boson, with 500 fb −1 of integrated luminosity shared between two beam polarization configurations at a centre-of-mass energy of 500 GeV. Other studies on this topic include Refs. [3][4][5][6][7][8][9][10][11][12][13][14][15][16][17].
Improving on the anomalous coupling description, we parametrize deviations from the standard model in top-quark pair production using a broad set of dimension-six effective operators. We include all ten dimension-six operators of the so-called Warsaw basis [18] involving a top quark and interfering with the resonant standard-model e + e − → tt → bW +b W − amplitudes, at leading order and in the limit of vanishing bottom-quark mass. This set contains four-fermion operators that are are absent in anomalous coupling descriptions as well as the CP-violating components of top-quark electroweak dipole operators. Four-fermion operators with a scalar or tensor Lorentz structure are treated separately. Various observables are discussed, in particular, the statistically optimal observables defined on the fully differential bW +b W − final state. They form a discrete set exactly sufficient to maximally exploit the information contained in distributions. For simplicity, the narrow top-quark width approximation and a vanishing bottom-quark mass are used in their definitions. The impact of non-resonant and higher-order corrections or detector effects should be determined before a comparison with real data. No major obstacle seems to prevent the achievement of those tasks. A detailed study of the detector response relying of full simulation will be presented elsewhere (see also Ref. [19]). We have extended the existing implementation of top-quark electroweak operators at next-to-leading order (NLO) accuracy in QCD [20] that was already available in the MG5_aMC@NLO software suite [21] to include four-fermion and CP-violating electroweak dipole operators. Prediction at that order, matched to parton shower, and including off-shell top-quark effects are thus made Figure 1. Tree-level diagrams contributing to the e + e − → bW +b W − production at lepton colliders: (a) the top-quark pair production through a s-channel Z boson or photon exchange, (b) representative diagram for single top-quark production e + e − → tbW − . available for these operators in the e + e − → bW +b W − process.
The impact of runs at various centre-of-mass energies and for several beam polarizations is examined. We derive global constraints on the whole ten-dimensional effectivefield-theory parameter space considered for different collider programmes. A special focus is devoted to two benchmark run scenarios covering the ranges of possibilities contemplated by future linear colliders, with runs at centre-of-mass energies of 500 GeV and 1 TeV and P (e + , e − ) = (±30%, ∓80%) beam polarizations for the ILC [22,23], and 380 GeV, 1.4 TeV and 3 TeV runs with P (e + , e − ) = (0%, ∓80%) beam polarizations for CLIC [24]. Circular lepton collider could also access top-quark pair production, collecting for instance 1.5 ab −1 at a centre-of-mass energy of 365 GeV, in addition to 200 fb −1 at the top-quark pair production threshold, without beam polarization [25]. We will also briefly discuss this scenario.
This paper is organized as follows. Top-quark production at lepton colliders is introduced in Sec. 2. Section 3 describes our effective-field-theory setup. Various observables are then discussed in Sec. 4, together with their sensitivity to operator coefficients. Statistically optimal observables are treated in a separate Sec. 5. The global reach of future lepton collider is then finally presented in Sec. 6. Our main results appear in Figs. 23, 24, and 25 for the three benchmark run scenarios considered. Comparisons with existing constraints and various HL-LHC prospects are provided Sec. 7. A few appendices include additional material, notably a conversion of our results into the effective-field-theory conventions established by the LHC TOP WG [26]. Useful computer codes and numerical results are made available at https://github.com/gdurieux/optimal_observables_ee2tt2bwbw.

Top-quark production at lepton colliders
In the standard model, lepton colliders primarily produce top quarks in pairs through a schannel Z boson or photon, as pictured in Fig. 1(a). A number of other processes, including single top-quark production illustrated in Fig. 1(b), also contribute to the bW +b W − final state. Although certain regions of the bW energies and invariant masses are enriched in double-and single-resonant processes [27,28], a clean separation is generally not achievable. It is therefore in principle preferable to consider the inclusive e + e − → bW +b W − process. Bound-state effects that significantly enhance the cross section in the threshold region are not included. Figure 2 displays the e + e − → tt and e + e − → bW +b W − production cross sections as functions of the centre-of-mass energy. Those results, accurate to next-to-leading order in QCD, are obtained with MG5_aMC@NLO [21]. The significant enhancement occurring at threshold is not accounted for. Two beam polarizations are chosen for illustration, with either 80% left-handed or 80% right-handed electrons. 1 The left-handed polarized electron beam leads to a significantly larger tt production cross section. The enhancement is even more pronounced for single top-quark production, as the neutrino-exchange diagram in Fig. 1(b) is absent for a right-handed electron. The pair production process is seen to provide the dominant contribution to e + e − → bW +b W − production for centre-of-mass energies below about 1 TeV. At higher energies, single top-quark production overtakes the s-channel pair production whose rate approximately falls off as 1/s. Single and pair production contributions have comparable magnitudes at about √ s 3 TeV. On the other hand, the bW +b W − production remains measurable below the pair production threshold down to √ s 300 GeV.

Top-quark effective field theory
We adopt an effective-field-theory approach to deviations from the standard model in topquark interactions. Remarkably, it is able to parametrize systematically the theory space in direct vicinity of the standard model, provided new states are not directly producible. Unlike anomalous couplings, it also preserves -by construction-the full standard-model gauge symmetry and constitutes a proper quantum field theory whose predictions are im- 1 Polarized positron beams are envisaged in the baseline ILC project, with relatively modest polarization (30% at 500 GeV, 20% at 1 TeV). Using the P (e + , e − ) = (+, −) and (−, +) configurations, the effective electron polarization reaches 90%, enhancing the effect observed in Fig. 2. As the degree to which the positron beam can be polarized depends on √ s, positron polarization is not considered in this figure. provable perturbatively, order by order. Importantly, its systematic character is retained only when all operators contributing to the studied process are simultaneously considered, up to a given order in the effective-field-theory expansion counted in powers of 1/Λ. Constraining effectively all directions in this sizeable parameter space requires the combination of various measurements. Performing global analyses is not only required but also permitted when using an effective field theory which is able to consistently make prediction in various sectors. Although more modest objectives are to be addressed first, a combination of measurements involving the Higgs boson, top and bottom quarks could ultimately be performed in the very same framework.

Operators
In this work, we limit ourselves to effective operators involving at least a top quark. Although other operators could also contribute to the e + e − → tt → bW +b W − process we study, they can presumably be constrained sufficiently well in other processes to have only a small impact on the marginalized bounds in the space of top-quark operator coefficients.
In terms of physical eigenstates, we define the fermionic gauge eigenstate out of which the gauge-invariant operators are constructed as where V CKM and V PMNS are respectively the Cabibbo, Kobayashi, Maskawa [29,30] and Pontecorvo, Maki, Nakagawa, Sakata [31][32][33] mixing matrices. In this work, we approximate both of them by unit matrices. Fermionic mass and gauge eigenstates are therefore not distinguished. Where they are unspecified, the generation indices of fields and operator coefficients will be set to '3' for quarks and '1' for leptons. We list, in their flavour-generic form, the operators of the chosen basis that affect the top-quark interactions at leading order. Given that the parity of an operator dimension is that of (∆B − ∆L)/2 [34], all operator conserving baryon and lepton numbers are of even dimension. We restrict ourselves to dimension-six operators and rely on the so-called Warsaw basis [18] (see also Refs. [35,36]), with normalizations convenient for our specific application. The correspondence between our conventions and the standards established within the LHC TOP Working Group [26] is detailed in Appendix E. Two-fermion operators affecting top-quark interactions have vector, tensor, or scalar Lorentz structures: O uZ ≡ s W c W (O uW − O uB ) combinations respectively give rise to a tensor coupling of the photon and Z boson to up-type quarks. In order to satisfy C uW O uW + C uB O uB = C uA O uA + C uZ O uZ , the corresponding operator coefficients are C uA ≡ C uW + C uB and C uZ = (c 2 W C uW − s 2 W C uB )/s W c W , where we have used the s W , c W shorthands for the sine and cosine of the weak mixing angle. Additionally, the O 3 ϕq and O uW operators also modify the interactions of the top quark, left-handed bottom quark and W boson. The O ϕud and O dW operators give rise to interactions between the top quark, right-handed bottom quark, and W boson. In the massless bottom-quark limit we use, these last two operators do not appear in interferences with standard-model amplitudes.
The two-quark-two-lepton operators of the Warsaw basis affecting top-quark interactions can also be grouped according to their Lorentz structures: As for the two-quark operators, we define the combinations O ± lq ≡ (O 1 lq ± O 3 lq )/2 and C ± lq = C 1 lq ± C 3 lq . The O ± lq operators respectively give rise to interactions between downtype quarks and charged leptons, and up-type quarks and charged leptons. Because of their chirality structures, the tensor and scalar operators above do not lead to amplitudes interfering with standard-model ones in the limit of vanishing lepton masses. All the fourfermion operators above but O ledq contribute at the Born level to the e + e − → tt process (see Fig. 3(a)). The O 3 lq , tensor and scalar operators also give rise to single top-quark production (see Fig. 3(b)) and t → b + ν decay (see Fig. 3(c)).
By convention, our effective Lagrangian includes the Hermitian conjugate of all operators, even though the flavour-diagonal component of some of them are already Hermitian: . This for instance compensates for the factors of 1 2 appearing in front of vector four-fermion operators. The energy scale Λ is conventionally set to 1 TeV. We treat the coefficients of the O ϕud , tensor (O uG excepted), and scalar operators as complex. Their imaginary parts produce CP-violating effects and have no interference with the standard model, in motion-reversal-even observables like total rates, at leading order, and in the V CKM = I approximation we use.
For convenience, we distinguish the real and imaginary parts of the weak dipole operator coefficients as two different real degrees of freedom: The different parity transformation properties and sensitivities of operator combinations featuring vector and axial-vector quark currents also motivate us to define: When focusing on operators that appear in top-quark pair production at the linear 1/Λ 2 level and at leading order, one counts 8 CP-conserving and 2 CP-violating parameters: We will mostly focus on these, discussing also the sensitivity to four-fermion scalar and tensor operators O S,T lequ . Note that the linear dependence on C ϕq operators drops out in the differential t → bW branching fraction in the narrow top-quark width approximation. The expressions of anomalous vertices in terms of effective-field-theory coefficients are provided in Appendix A.

Specific models
The effective field theory described above can be matched to specific new-physics models. Effective-operator coefficients then become functions of the underlying model parameters which therefore inherit their constraints. Different patterns of correlations between operator coefficients are produced depending on the model. Any evidence for non-vanishing operator coefficients can thus also point at particular extensions of the standard model. For illustration, we consider in this section two kinds of models: the first one produces two-quark operators only and the second one also yields two-quark-two-lepton operators with vector Lorentz structures. Scalar and tensor four-fermion operators could be obtained from the exchange of heavy scalars or vector leptoquarks (after Fierz rearrangement).
Two-quark operators like O 1,3 ϕq and O ϕu can be generated at tree level by mixing of standard-model particles with new fields of identical quantum numbers: W , Z , or heavy quarks. The O uW and O uB operators are in general generated at the loop level in scenarios like two-Higgs-doublet or supersymmetric models.
Let us consider, for illustration, the mixing of new vector-like quarks with the third generation. The complete matching for such scenarios has been carried out in Ref. [37]. A singlet U with quantum numbers identical to that of u could mix with the third-generation quark doublet via a λŪ R q ϕ interaction. Integrating out U then gives So limits on C − ϕq /Λ 2 can be turned into limits on λ 2 /M 2 U . Direct LHC constraints on M U are around 1.2 TeV regardless of λ [38]. Together with a limit of the order of C ϕq /Λ 2 0.2 TeV −2 which can realistically be obtained at future lepton colliders as we will see below, this would imply λ 1.1.
Alternatively, a SU (2) L doublet T = (X, U ) with hypercharge 7/6 could mix with the third-generation quark singlet via λT u ϕ. In this case, a different operator is generated: (3.4) Again, limits on C ϕu /Λ 2 can expressed in terms of λ 2 /M 2 U . Furthermore, the pattern of deviation yields information about the underlying new physics. Direct limits on M U for a SU (2) L doublet are of the order of 850 GeV [38]. Again, combined with C ϕu /Λ 2 0.2 TeV −2 , this would constrain λ 0.54.
Two-quark-two-lepton operators of vector Lorentz structure (like O 1,3 lq , O lu , O eq , or O eu ) could for instance be generated in models featuring new heavy gauge bosons, such as a Z . In non-flavour-universal scenarios, couplings to the third generation could be enhanced. Randall-Sundrum (RS1) models of a warped extra dimension in which standardmodel fermions and gauge fields propagate [39,40] belong to this category. Because it is localized near the TeV brane, the top-quark has its couplings to the KK modes of the electroweak gauge bosons enhanced by a factor of O(ξ), where ξ ≡ √ kπr c 6. On the contrary, the light fermions are localized near the Planck brane so that their couplings are suppressed by O(ξ −1 ).
The electroweak gauge group in the bulk is SU (2) L × SU (2) R × U (1) X . So we will consider the first KK mode of photon, Z, and Z X -which is the combination of U (1) R,X orthogonal to U (1) Y -denoted respectively as A 1 , Z 1 and Z X1 . The couplings of these three modes to the third-generation t L,R and b L are enhanced. Considering the benchmark model depicted in appendix A.3 of Ref. [40], i.e setting g L = g R , c t R = 0, c t,b L = 0.4, the couplings of the three KK modes to the SM fermions can be written as where s W = g X /g Z . Once the KK modes are integrated out, at leading order, the effective Lagrangian is The four-fermion operators involving only light fermions are suppressed by O(ξ −2 ) and negligible. We focus on the operators that involve two light fermions and two top quarks, for which the suppression factor ξ −1 on the light fermion side cancels the enhancement factor ξ on the top-quark side. Using M A 1 ,Z 1 = m KK and M Z X1 0.981m KK , and inserting the values of κ X f for electron and top-quark fields, we find Indirect constraints on the KK mass can thereby be derived. Limits of the order of 10 −1 , 10 −3 and 10 −4 -which can be obtained at circular, ILC-and CLIC-like colliders, as we will see-would respectively translate into m KK 0.5, 5 and 15 TeV. Note however that the generated two-fermion operator coefficients are not negligible. The modification if light-fermion couplings are suppressed, and can be captured by a redefinition of the oblique parameters [39], so we will not consider them here. We need to take into account the contribution to Ztt couplings, which correspond to the operators O − ϕq and O ϕu . It is interesting to ask which kind of operator better probes the proposed scenario, at a given collider. The four-fermion operators describe the underlying process e + e − → Z → tt. As mentioned above, this is neither suppressed nor enhanced by ξ, and its amplitude is of order s/m 2 KK . The vertex operators, on the other hand, describe the process e + e − → Z → Z → tt through ZZ mixing, which is of order ξm 2 Z /m 2 KK . Furthermore the Z tt vertex is enhanced by a factor of ξ. Altogether, this amplitude is of order ξ 2 m 2 Z /m 2 KK . Therefore the relative contributions of two-and four-fermion operators depend approximately on the relative size of collider energy √ s and ξm Z . As a comparison, in the same scenario described above, we find Which would translate into m KK 4 TeV for C ϕq,u /Λ 2 0.2 TeV −2 . Of course, in practice both effects should be accounted for simultaneously and a global analysis performed. The top-quark also plays a distinct role in composite Higgs models. Pair production measurements at lepton colliders are therefore especially sensitive to such scenarios. A dedicated discussion will be presented elsewhere [41].

Validity
The use of effective field theories relies on a low-energy decoupling theorem [42]. It states that, in unbroken gauge theories, the effects of heavy fields on phenomena observed at energies scales E much smaller than their masses M are suppressed by powers of E/M . In this low-energy limit, these effects can be parametrized by a tower of higher-and-higher dimensional operators suppressed by higher-and-higher powers of 1/M . Retaining only the operators of lowest dimensions is then justified when E/M 1. In a bottom-up approach that does not assume some specific heavy new physics, the operator coefficients C and mass scale Λ stand for unknown combinations of couplings and masses. They always appear as C/Λ 2 ratios (for dimension-six operators), on which the only model-independent information arises from the experimentally imposed constraints. The validity of the low-energy limit is then rather intangible: it requires the physical scale M of the underlying theory to be significantly higher than the energies E probed in the process described through our effective field theory. Without explicit model or power counting, this condition cannot be translated in terms of C and Λ, and no statement about the relative magnitude of different operator coefficients -of identical or different dimensioncan be made a priori either. As we will not consider the dependence on operators of higher dimensions, our results will only be interpretable in models where dimension-six operators provide the leading contributions to the observables considered.
Under the assumption that higher-dimensional operators are subleading, one may examine what truncation of the series in powers of dimension-six operator coefficients is sensible. The expansion of an observable in dimension-six operator coefficients can be expected to contain higher-and-higher powers of CE 2 /Λ 2 where, again, E is the characteristic energy scale of the process considered. For tree-level operator insertions and a coefficient normalization that is natural to the observable considered, numerical prefactors in this series can naively be expected to be of order one, schematically: More moderate growths with energy are also possible, especially for the linear terms which arises from interferences between effective-field-theory and standard-model amplitudes. This first term roughly dominates the expansion when CE 2 /Λ 2 1. Given the experimental bound on C/Λ 2 and the energy E of the process considered, one can explicitly check whether this condition is satisfied. If it is not, higher powers of C/Λ 2 should also be included. Note that dimension-eight operators in principle start contributing at order 1/Λ 4 . Note also that the renormalizability of quadratic dimension-six contributions in general requires counterterms from dimension-eight operators. Quantum perturbativity restrictions on the dimension-six effective field theory can also be derived by considering the insertion of more-and-more operators in higher-and-higher numbers of loops. For one additional insertion in each loop and a suitable coefficient normalization, such a series contains higher-and-higher powers of CE 2 /(4πΛ) 2 . Perturbativity is therefore lost when CE 2 /Λ 2 approximately exceeds (4π) 2 .
At lepton colliders, one can expect precision measurements at each centre-of-mass energy (which constitutes the characteristic scale of a production process) to reach the percent level. The combination of such percent-level measurements, provided they are sufficiently complementary, should be able to constrain all directions of the effective-fieldtheory parameter space at the CE 2 /Λ 2 < 10 −2 level. Terms beyond the leading one are then naively expected to induce only percent-level corrections to the constraints set with a linearised effective field theory. Complications invalidating this general reasoning are however bound to arise in some specific cases. In particular, some dimension-six operators are known to have (highly) suppressed interferences with the standard model. Helicity selection rules can for instance cause such suppressions [43]. As mentioned earlier, they also occur for operator containing a tensor or scalar lepton current, involving a right-handed b-quark, or violating CP. The dominant contributions of such operators to observables can then arise from the square of amplitudes in which they are inserted once. In practice, we will focus mostly on linear effective-field-theory dependences and examine the quadratic dimension-six contributions to ensure they are subleading. The quadratic dependence of scalar and tensor four-fermion operators will be discussed briefly.

Observables and sensitivities
We examine the sensitivity of several observables to the operators affecting top-quark pair production at lepton colliders. To efficiently constrain all directions in the multidimensional space of operator coefficients, various observables are to be combined. Runs with different beam polarizations and centre-of-mass energies provide complementary handles.

Cross section and forward-backward asymmetry
Definitions Let us consider first the simplest observables one can define in the e + e − → tt process, namely the total cross section σ and forward-backward asymmetry A FB which is defined as follows: where θ t is the angle between the positron and top-quark momenta in the centre-of-mass frame.

Computation
We computed the standard-model, linear, and quadratic dependences of the total and forward-backward cross sections both analytically at leading order, and using MG5_aMC@NLO [21] at next-to-leading order in QCD, for the various initial-state helicities. For illustration, the leading-order total and forward-backward e + e − → tt cross sections, for unpolarized beams and √ s = 500 GeV, are displayed in Table 1. The linear effectivefield-theory dependences computed at NLO in QCD are provided in Appendix C.
As can be seen in Fig. 4 for total (left) and forward-backward integrated (right) cross sections, the NLO QCD k-factors in the standard model and in the linearised effective field theory are fairly similar, diverging from each other mostly at higher centre-of-mass energies. The ratios of those two types of contributions, which assess the sensitivity to operator coefficients, are therefore only marginally affected by QCD corrections. In the following, central values will always be assumed to confirm the standard-model hypothesis, and deviations will be considered at leading order everywhere but in Sec. 5. Table 1. Leading-order dependence on the effective operator coefficients of the unpolarized total and forward-backward e + e − → tt cross sections at √ s = 500 GeV.   The bands' thickness covers QCD renormalization scale variation between m t /2 and 2m t .  Sensitivity We define the sensitivity of an observable o to an operator coefficient C i as its normalized variation in that direction, around the standard-model point: The scale Λ, conventionally set to 1 TeV as noted earlier, is absorbed into the definition of o i , o ij , etc. The left panel of Fig. 5 shows the sensitivity of the cross section to operator coefficients, as a function of the centre-of-mass energy, for a mostly left-handed electron beam polarization P (e + , e − ) = (+30%, −80%). It tends to a constant value at high energies for the two-quark operators: C A ϕq , C V ϕq , C R uZ and C R uA . This behaviour can be understood given that the ϕq operators induce ttZ couplings which scale as v 2 /Λ 2 once the two Higgs fields they contain condense to their vacuum expectation value. The sensitivity of the cross section to the O V ϕq operator actually slightly decreases with energy, as 1 + 2m 2 t /s. On the other hand, the two uA and uZ electroweak dipole operators generate three-point interactions scaling as Ev/Λ 2 , where E is an energy scale characteristic of the momentum transfer in the associated vertex. Their interference with standard-model amplitudes of identical top-quark helicities however requires a flip of chirality along the quark line, and thus a top-quark mass insertion. 2 The resulting linear effective-field-theory contributions therefore scale with energy exactly as the standard-model cross section and the sensitivity tends to a constant. As will be discussed below, a sensitivity to the dipole operators that grows with energy can be recovered through the interference of different helicity amplitudes once the angular distributions of the top-quark decay products are considered. The sensitivity of the cross section to four-fermion operator coefficients C V lq , C A lq , C V eq , C A eq shows the naive s/Λ 2 increase with energy expected from dimensional analysis (see dashed black line). The constraints on those operators therefore highly benefits from increased centre-of-mass energies.
2 It is formally seen that none of the individual helicity amplitude squared provided in Eq. (4) of Ref. [5] leads to a Re{F * 1V,1A F2V } term proportional to γ ≡ √ s/2mt.
Individual one-sigma limits from cross section Individual one-sigma limits from forward backward asymmetry The forward-backward cross section also has an enhanced sensitivity to the axial-vector combinations of operators, 3 while the total cross section is more sensitive to vector operators. This is especially true at lower energies where the sensitivity of the total cross section to the O A ϕq , O A eq , and C A lq operators suffers from a so-called p-wave suppression and falls off as β ≡ (1 − 4m 2 t /s) 1/2 . In the forward-backward asymmetry, both the standard-model and linear effective-field-theory dependences are proportional to β so that this suppression drops out in their ratio.
Individual statistical constraints deriving from the measurements of cross sections and forward-backward asymmetries are displayed in Fig. 6 as functions of the centre-of-mass energy. They are arbitrarily normalized to an integrated luminosity times efficiency of 1 ab −1 . Note however that, at linear colliders, the instantaneous luminosity which can be achieved scales approximately linearly with the centre-of-mass energy, while it falls off as the fourth power with the centre-of-mass energy at circular lepton colliders for a constant power of synchrotron radiation emission. Unlike the sensitivity, these idealised individual limits also account for the statistical precision to which cross sections and forward-backward asymmetries can be measured. Quite naturally, the operators whose sensitivity does not grow with energy are more efficiently constrained at lower centre-of-mass energies, where the top-quark pair production cross section is larger. For those, the optimal centre-of-mass energy lies roughly between 400 and 600 GeV.
Complementarity With unpolarized beams, the combination of cross section and forward-backward asymmetry measurements allows to simultaneously constrain pairs of operator coefficients, as illustrated in Fig. 7. Runs with two different beam polarizations effectively duplicate the number of observables. Polarization was shown to effectively provide separate sensitivity to the photon and Z-boson form factors in Refs. [1,2]. Similarly, in an effective field theory, dipole operator coefficients C R uZ and C R uA can be disentangled very effectively by taking data in two different beam polarization configurations. The combination of the cross section and A FB measurements with unpolarized beams are largely degenerate in this two-dimensional parameter subspace, see Fig. 8 (left). The combination of measurements with different beam polarizations, on the other hand, yields the tight constraint shown in Fig. 8 (right).

Top-quark polarization
We have seen in the previous section that the sensitivity to the electroweak dipole operator coefficients C uA , C uZ of the cross section and forward-backward asymmetry is approximately constant as a function of centre-of-mass energy. To achieve a sensitivity that grows with energy we must consider the interference between amplitudes with top quarks of different helicities. This can therefore only be observed through observables incorporating top decay product distributions. Statistically optimal observables based on the e + e − → tt → bW +b W − kinematics as well as on the W polarizations were already shown to exhibit such a sensitivity growing with the centre-of-mass energy in Ref. [4]. This tech- nique will be revisited in Sec. 5. We examine in this section the sensitivity of a number of alternative observables. One could study the polarization of the top quark along its direction of motion in the centre-of-mass frame, by examining the angular distribution between one of the top-quark decay products in its rest frame. This so-called helicity angle distribution takes the form where P is the polarization and α i is the so-called analysing power of the decay product i. The charged lepton and down-type quark arising from the W decay are known to have the largest α i . At leading order and in the absence of C I uZ,uA and C S,T lequ operator coefficients, P is however not independent of the forward-backward production asymmetry. In terms of tt helicity amplitudes (see e.g. Refs. [5,44]), the forward-backward asymmetry is sensitive to the In the standard model, however, |++| 2 = |−−| 2 . This remains true when introducing CP-conserving dipole operators, or two-and four-fermion operators having (axial) vector Lorentz structures.
Generalisations of the W helicity fractions (see Sec. 4.4) have been proposed in Ref. [45]. They are based on the definition of two additional axes in the top-quark rest frame -besides the direction of motion of the W boson-with respect to which the angle of the charged lepton momentum in the W rest frame could be measured. For this purpose, it is prescribed to use a reference direction along which most of the top-quark polarization lies. Reference [44] demonstrated that a convenient such direction is that the incoming positron for the top and that of the incoming electron for the anti-top (in the respective top and anti-top rest frames). One can then define two new axes,ê ×Ŵ andŴ × (ê ×Ŵ ), from the directions of the W boson and electron (positron) beam in the top (anti-top) rest frame. One can for instance construct asymmetries based on the sign of the cosine of the angle between either of these directions and the direction of the charged lepton arising from the leptonic W decay measured in that W rest frame. Inspired by this proposal but aiming to obtain sensitivity to the top-quark polarization instead of that of the W , we define normal and transverse axes in the centre-of-mass frame: N ≡t ×ê andT ≡t ×N from the direction of motion of the (anti-)topt and that of the electron (positron) beamê. Being orthogonal tot, those vectors are not affected by a subsequent boost in the (anti-)top rest frame. Observables generalizing P can then be constructed from the distribution of the angles betweenN orT and one of the top-quark decay product, in the top-quark rest frame. The direction of the charged lepton arising from a semi-leptonic top-quark decay will be employed in the following. Asymmetries based on the sign of the cosine of either of these angles will be named normal and transverse polarization asymmetries, A N and A T .
In the same format as Fig. 6, we compare in Fig. 9 the one-sigma limits obtained from measurements of the forward-backward production asymmetry (solid line), the transverse polarization asymmetry (dashed line), and the statistically optimal observables (dotted line) on the coefficients of the dipole operators C R uA and C R uZ . As mentioned earlier, the standard helicity angle asymmetry is fully degenerate with the forward-backward production asymmetry A FB . Here again, a constant integrated luminosity times efficiency of 1 ab −1 is assumed at any given centre-of-mass energy. The left and right panels respectively assume mostly left-handed and mostly right-handed electron beam polarizations. The effective-field-theory dependences of the top-quark width and of its decay amplitudes have been included. At low energy, the transverse polarization asymmetry yields similar limits as A FB , but its added value becomes clear at high energy. The sensitivity of A FB is approximately constant over the √ s range considered here (see right panel of Fig. 5). Therefore, with the cross section falling as 1/s and the luminosity assumed constant, the Individual one-sigma limits on C I uA and C I uZ L=1 ab −1 P (e + ,e − )=(+30%,−80%) e + e − → tt → lepton plus jets from optimal observables from A Re 500 1000 3000 Individual one-sigma limits on C I uA and C I uZ L=1 ab −1 P (e + ,e − )=(−30%,+80%) e + e − → tt → lepton plus jets from optimal observable s from A Re 500 1000 3000 10 −2 10 −1 Figure 10. Individual limits on the imaginary parts of the dipole operator coefficients C I uA and C I uZ from measurements with P (e + , e − ) = (−30%, +80%) and (−30%, +80%) beam polarizations (left and right panels, respectively). The limits deriving from A Re measurements (solid lines) are compared to that of optimal observables defined in Sec. 5. A data sample of 1 ab −1 is assumed at centre-of-mass energies ranging between the top-quark pair production threshold and 3 TeV. limits deteriorate strongly with increasing centre-of-mass energy. The sensitivity of the transverse asymmetry to dipole operators, on the other hand, increases with centre-ofmass energy. At high energies, both the sensitivity and the statistical uncertainty increase as √ s and balance each other. The individual limits thus become independent of √ s. For centre-of-mass energies above 1 TeV, the constraints derived from the transverse asymmetry are significantly stronger than those implied by A FB . At 3 TeV, they are an order of magnitude better. The optimal observables that will be introduced in Sec. 5 present a similar high-energy behaviour but perform better than the transverse polarization asymmetry at low energies.
Measurements of the transverse polarization asymmetry may add valuable information in a global fit of top-quark electroweak couplings. The information contained in the usual helicity angle asymmetry overlaps with that of the forward-backward asymmetry. The sensitivity of the transverse polarization asymmetry grows with the centre-of-mass energy and yields significantly tighter constraints for √ s above about 1 TeV.

CP-odd observables
Imaginary coefficients for the electroweak dipole operators O uZ and O uA (or O uW and O uB ) violate the combination of charge conjugation and parity symmetries (CP). Close-tooptimal observables specifically designed to test CP conservation [46] provide very precise constraints on these parameters [47]. Following Ref. [46], one defines first wheret (t) andê + are unit vectors pointing in the direction of the top (anti-top) and incoming positron beam momenta in the centre-of-mass frame. The unit vectorsl ± point in the direction of the charge lepton momenta arising from the W decay in the top and  [47]. The limits extracted from the A Re asymmetry are very similar to the limits obtained from the top and anti-top normal polarization asymmetries defined in Sec. 4.2, with a slight advantage for the A Re asymmetry. Both observables are indeed based on the same O Re ± kinematic functions. We therefore only discuss the A Re asymmetry.
The one-sigma individual limits on the imaginary parts of the dipole operator coefficients C I uA and C I uZ are presented as functions of the centre-of-mass energy in Fig. 10. As before, the integrated luminosity is fixed to 1 ab −1 to facilitate comparisons. The limits extracted from the A Re asymmetry are displayed together with those obtained with the optimal observables that will be defined in Sec. 5. Both are comparable at low centre-of-mass energy, but differ by up to a factor two between √ s = 1 and 3 TeV. This gain may arise from the higher top-quark spin analysing power of the charged lepton compared to that of the W boson (or b quark) that is accessible to statistically optimal observables defined on the bW +b W − kinematics. In both cases, the sensitivity grows with the centre-of-mass energy. At large energies and for a fixed integrated luminosity, the individual limits saturate to constants. These observables are quite specific to the imaginary part of the O uA and O uZ operators and the constraints they imply have little correlations with that of the CP-conserving operator coefficients.

Top-quark decay and single production
Some of the dimension-six operators that affect the top-quark couplings to the photon and Z boson also modify the tbW vertex. Among those, O uW and O 3 ϕq interfere with standard-model amplitudes in the vanishing b-mass limit. These two operator coefficients are constrained at the LHC in measurements of top-quark decay, single-top and associated ttV production (see for instance Ref. [59]).
In e + e − collisions, the O uW and O 3 ϕq operators affect top-quark pair production, single production, and decay. We compare in this section the sensitivity of the production and decay processes to the C uW operator coefficient. In the narrow top-quark width approximation, the dependence on O 3 ϕq drops out from the differential t → bW branching fraction. The e + e − → tt process is only sensitive to the difference of . We explore several ways to disentangle the contributions of O 1 ϕq and O 3 ϕq .

Transverse polarization asymmetry
The transverse polarization asymmetry of the top quark A T , introduced in Sec. 4.2, is sensitive to new physics in top-quark production. It may also be affected by new physics in top-quark decay since it relies on the distribution of the charged lepton produced in the t → W b, W → lν l decay chain.
W helicity fractions The helicity fractions of the W boson are two classical observables measured in top-quark decay. We denote θ * l the angle between the charged lepton momentum in the W -boson rest frame and the W -boson momentum in the top-quark rest Table 2. Sensitivities to the C R uW operator coefficient, artificially decomposed into production and decay components, and quoted in percent. A centre-of-mass energy of 500 GeV and the two P (e + , e − ) = (±30%, ∓80%) beam polarizations are considered. The uncertainties displayed are due to limited Monte Carlo statistics. A sensitivity compatible with zero, within uncertainties, is replaced by a dash. frame. Its distribution, serves to define the positive, negative and longitudinal W -boson helicity fractions of unit sum: F + +F − +F 0 = 1. In the following, we consider the asymmetry formed by positive and negative helicity fractions A W F B ≡ 3 4 (F + −F − ) extracted from a fit to the cos θ * l distribution. Leading-order standard-model estimates for A T and A W F B are presented in the first row of Table 2 for a centre-of-mass energy of 500 GeV and the two P (e + , e − ) = (±30%, ∓80%) beam polarizations. The remaining rows present the sensitivity of these observables to C R uW , artificially decomposed into components arising from top-quark production and decay, in the narrow width approximation. For the purpose of this table, the sensitivity of an observable o is simply defined as o(C = 1)/o(C = 0) − 1 and quoted in percent. The transverse polarization asymmetry has a marked sensitivity to C R uW . It arises dominantly from production. On the other hand, the sensitivity of the W helicity fractions to C R uW mostly arises from top-quark decay. For the centre-of-mass energy considered, it is smaller than the one achieved with the transverse polarization asymmetry.
Total width Measurements of the top-quark decay width are sensitive to dimension-six operators. Computing its linear dependence at NLO in QCD using with MG5_aMC@NLO [21] and the input parameters specified in Appendix C, we obtain: Central values, k-factors and uncertainties are displayed in the following format: Figure 11. One-sigma constraints on the C R uW and C 3 ϕq operator coefficients that would derive from a measurement of the top-quark width with 20, 40, or 80 MeV precision. The central value of the measurement is assumed to coincides with the SM prediction.
The scale uncertainty is computed from the running of α S (µ) between µ = m t /2 and 2m t .
The top-quark width has only a leading-order linear dependence on C 3 ϕq and C R uW operator coefficients. A small dependence on C R uG also arises at next-to-leading order in QCD. Tight constraints on this operator coefficient can however be obtained at the LHC, or from the associated production of a top-quark pair with a hard jet at a linear collider [60]. We therefore ignore this dependence. For constraints achievable at lepton colliders, the quadratic dependences on the coefficients which appear already at the linear order are subleading. Operators inducing a right-handed current or CP-violation only start contributing a the quadratic level.
A precise measurement of the top-quark width is possible at an e + e − collider by scanning the centre-of-mass energy through the top-quark pair production threshold. 4 Reference [62] demonstrated that a precise determination, simultaneous to that of the top-quark mass and strong coupling constant, can be obtained from a fit of the threshold line shape. A recent analysis estimates the statistical uncertainty obtainable with an integrated luminosity of 100 fb −1 to 21 MeV [63]. Theory uncertainties are however likely to dominate. For uncertainties of 20, 40, and 80 MeV and a standard-model central value, the regions of the parameter space spanned by the operator coefficients C R uW and C 3 ϕq allowed at the 68% C.L. are presented in Fig. 11. The constraint imposed by the width measurement effectively disentangles the coefficients of the O 1 ϕq and O 3 ϕq operators.
Single production Single top-quark production at e + e − colliders is also sensitive to modification of the tbW vertex. 5 At high energy, its cross section becomes comparable that of pair production. A dedicated analysis was presented in Ref. [66]. The limits on 4 A determination of the total width is also possible immediately below the tt threshold [61] or in the continuum well above the threshold [28]. 5 Single production through a eγ initial state could also be considered [64,65].  [67]. For each measurement the future lepton collider beam polarization configuration that yields the best limit has been chosen: P (e + , e − ) = (+30%, −80%) for the cross section measurements and the tt forward-backward asymmetry, P (e + , e − ) = (−30%, +80%) for the bb forward-backward asymmetry.
dimension-six operator coefficients are weak compared to the ones obtained from a study of top-quark pair production. Ideally, an analysis should treat the full e + e − → bW +b W − process, including dimension-six operator effects on both resonant and non-resonant components. Four-fermion operators should also be included. The statistically optimal observables we employ in this work could be extended to cover non-resonant contributions and enhance the sensitivity to charged current modifications. This is left for future work.

Bottom-quark production
Measurements in the e + e − → bb process can provide complementary constraints on several operators. The combination of tt and bb data can disentangle contributions from O 1 ϕq and O 3 ϕq operators. The tt production process constrains only the difference C 1 ϕq − C 3 ϕq , while bb data constrain the sum C 1 ϕq + C 3 ϕq . The combination of both types of measurements provides stringent constraints on both coefficients. Of course, a combined global fit of tt and bb data also increases the set of relevant operators. Two additional two-fermion operators of the Warsaw basis must then in principle be considered, O dW and O ϕd , plus three new four-fermion operators of vector Lorentz structure (O ld , O + lq , O ed ) which do interfere with standard-model amplitudes. The real and imaginary components of an additional scalar four-fermion operators O ledq do not.
A combined fit is beyond the scope of the present work, but it is instructive to consider a simple two-parameter fit of the coefficients C 1 ϕq and C 3 ϕq . Constraints of several origins are compared in Fig. 12. The red bands represent existing constraints from the characterization Table 3. Individual 68% C.L. limits on the scalar and tensor four-fermion operator coefficients obtained with an integrated luminosity of 500 fb −1 collected at √ s = 500 GeV. Following the ILC scenarios of Ref. [69], respectively 40% and 10% of the total luminosity is devoted to runs with each of the P (e + , e − ) = (−30%, +80%), (+30%, −80%) and P (e + , e − ) = (−30%, −80%), (+30%, +80%) polarization configurations. We assume A pol is measured in lepton-plus-jets events. A total efficiency to 20% is applied, including top-quark branching fractions and an estimate of the selection efficiency. The scale Λ is fixed to 1 TeV.
of the e + e − bb process at LEP and SLC. We consider two measurements. The first, in the left panel, is the combination of measurements from the four LEP1 experiments and SLD of the bb cross section [67]. 6 The second measurement, in the right panel, is the forwardbackward asymmetry of bottom quarks. The latter can be compared to Fig. 11 of Ref. [17]. The combination of LEP1 measurements yields a stronger constraint than the single A FB bb measurement considered there.
Two additional bands in Fig. 12 indicate the constraints that can be expected from measurements at the ILC. The green shaded band shows the limit expected from bb production at the ILC at √ s = 250 GeV, based on the analysis of Ref. [68]. The constraint from the cross section is similar in strength to the equivalent result from LEP1. The sensitivity is practically constant as a function of the centre-of-mass energy and the impact of the cross section, which is nearly four orders of magnitude larger at the Z-pole than at 250 GeV, roughly cancels the effect of the much greater luminosity at the ILC. The constraint from A FB , on the other hand, is greatly improved by ILC data. In a global fit, this complementary information is important to simultaneously constrain all operator coefficients. With higher centre-of-mass energies, future lepton colliders would also be much more sensitive to four-fermion operators.
The e + e − → bb data provide very tight constraints on the O ϕd ≡ This observation can be related to the results in Ref. [68] using the relations between the operator coefficients and the left-and right-handed couplings of the b-quark to the Z-boson they define there: We see that both studies indeed find that the right-handed coupling is improved considerably, while for the left-handed coupling LEP1 and ILC constraints are of comparable strength.
The blue band indicates the limit that is obtained from tt production at √ s = 500 GeV. These bands cross the e + e − → bb bands at a right angle. A combined fit is thus expected to yield a tight constraints on both operator coefficients.

Observables for scalar and tensor operators
The scalar and tensor four-fermion operators O S lequ and O T lequ present a distinctive Lorentz structure. As mentioned earlier, they do not interfere with standard-model amplitudes in the limit of vanishing lepton masses. For the range of energy and initial state polarizations we consider, we find the difference A pol = P t − Pt of the polarization of the top and antitop quark (see Sec. 4.2) is sensitive to both operators. In a lepton-plus-jets sample, both polarizations are measured in a straightforward fashion through Eq. (4.2). The observable A pol vanishes in the SM and is specific to the scalar and tensor operators: it has little or no sensitivity to any of the other operators considered. Table 4. Individual limits on the square of the Wilson coefficients of the scalar and tensor operator coefficients at √ s = 3 TeV. A pol is measured in lepton+jets events in a data sample with an integrated luminosity of L = 3 ab −1 . A selection efficiency of 20% is applied. For comparison to the ILC scenario, a 30% positron polarization is assumed and the sample is divided among the four configurations as in Table 3 The sensitivity to the scalar and tensor operator moreover increases in runs with electron and positron beam polarizations of the same sign. In Fig. 13, the sensitivity of A pol to the O S lequ and O T lequ operators at a centre-of-mass energy of 500 GeV is represented for four different initial-state polarization configurations. The curves labelled e − L e + R and e − R e + L represent the opposite-sign configurations that are usually considered, with P (e + , e ) = (+30%, −80%) and P (e + , e − ) = (−30%, +80%). Two further curves, labelled as e − L e + L and e − R e + R represent same-sign configurations with P (e + , e − ) = (−30%, −80%) and P (e + , e − ) = (−30%, −80%). Clearly, the same-sign configurations e − L e + L and e − R e + R enhance the sensitivity to these operators significantly. The tensor operator has a larger impact on A pol for all scenarios considered here.
To get a grasp of the √ s dependence of the sensitivity we consider 3 TeV operation under the same conditions. The CLIC baseline design does not envisage positron polarization. There is however no technical impediment to positron polarization at high energy. We therefore present the sensitivity plots at √ s = 3 TeV under the same conditions as the ILC in Fig. 14. As already observed for the other four-fermion operators, the sensitivity increases strongly with centre-of-mass energy (note the different range on the x-axes between Figs. 13 and 14).
Operations with same-sign polarizations help constraining the scalar and tensor fourfermion operator coefficients. The ILC operating scenarios envisage a fraction of the integrated luminosity to be collected in the same-sign configurations. At √ s = 500 GeV, Ref. [69] equally splits 80% of the integrated luminosity between the P (e + , e − ) = (+30%, −80%) and (+30%, −80%) polarizations. The remaining 20% are shared among P (e + , e − ) = (+30%, +80%) and (−30%, −80%) configurations. We provide individual 68% C.L. limits on the scalar and tensor operator coefficients, in Table 3, assuming a total integrated luminosity of 500 fb −1 . Statistical uncertainties are based on 20% of the tt sample, to take into account the branching fraction of the lepton-plus-jets final state and an estimate of the selection efficiency.
The results in Table 3 indicate that the same-sign configurations can indeed offer quite powerful constraints. The higher sensitivity compensates for the smaller integrated luminosity. Individual limits on |C S lequ | 2 and |C T lequ | 2 approximately reach the 10 −3 level for all configurations. As for the other four-fermion operators, the sensitivity dramatically improves with the centre-of-mass energy. Individual constraints obtained with 3 ab −1 of integrated luminosity collected at a centre-of-mass energy of 3 TeV are displayed in Table 4 and reach the 10 −6 level.

Statistically optimal observables
Let us now examine statistically optimal observables exploiting the full bW +b W − kinematics, still focusing on resonant production, treating the top quarks in the narrow width approximation and in the m b /m t → 0 limit. Their analytical construction is based on the decomposition of the differential e + e − → tt → bW +b W − cross section in terms of helicity amplitudes, carried out for instance in Ref. [5]. We extended it to include the dependence on four-fermion operators. The same technique was already employed in the context of top-quark pair production at lepton colliders in Ref. [4,11,15,16]. Different differential distributions were nevertheless employed: including also the W polarization information [4], the kinematic information about the W decay products [16], or nothing else than the energy and production angle of one final-state charged lepton or bottom quark [11,15].
Statistically optimal observables [4,70] are constructed to maximally exploit the available differential information and extract the tightest constraints on parameters whose dependence is expanded to linear order only. The total rate information is employed too, in the following. Perfect optimization naturally requires a model that truly describes the data. For a differential distribution across the phase space Φ given by the observables maximizing the constraints on the {C i } parameter space are shown to be the average values of O i = n dσ i dΦ dσ SM dΦ where n is the number of events observed. They can be computed asŌ where L is the total integrated luminosity and an can be introduced to effectively account for finite efficiencies. Defining their sensitivity to operator coefficients and the covariance matrix on the extracted C i are given by In most of our discussion, we will only retain the zeroth order in C k of these quantities. We show in Fig. 15 the S O i i sensitivities for both mostly right-handed and mostly lefthanded polarized electron beams. Note these sensitivities are not necessarily maximized   Figure 15. Sensitivity of each statistically optimal observable to the corresponding operator coefficient. Note that these observables do not necessarily have maximal sensitivities but rather, as a set, induce minimal statistical uncertainties on the coefficient determination.
by the statistically optimal observables which rather minimize (the determinant of) the covariance matrix. Even though such observables can be used to constrain the C I uZ,A operator coefficients, the corresponding sensitivities could not be displayed in Fig. 15 since the standard-model values of these observables σ i vanish. In contrast to that of the total and forward-backward cross sections (see Fig. 5), note the sensitivities of the statistically optimal observables to dipole operators slowly grow with √ s in the range shown. Beyond the energies displayed, they actually start growing quadratically with the centre-of-mass energy, like the four-fermion operators. This can be understood by examining the √ s dependence of d ij and σ i . In the large centre-of-mass energy limit, dσ SM /dΦ scales as 1/s. Both dσ i /dΦ and σ i ≡ dΦ dσ i /dΦ tend to constants for four-fermion operators while they respectively scale as 1/ √ s and 1/s for dipole operators, given that the former scaling arises from terms having an azimuthal angle dependence which vanishes upon phase-space integration. Then, d ij tends to a constant for dipole operators and grows like s for fourfermion ones, while σ i scales like 1/s for the former and tends to a constant for the latter. The ratio of these two quantities therefore behaves as s in both cases.
Beside sensitivities, it is even more instructive to look at the centre-of-mass energy dependence of the individual one-sigma statistical limits on the C i operator coefficients. They are given by (V −1 | ii ) −1/2 = ( L d ii ) −1/2 . For definiteness and as in the previous sections, we normalize them to an integrated luminosity times efficiency of 1 ab −1 . As seen in Fig. 16, a targeted constraint on the four-fermion and C I uZ,A operators can be obtained with lower luminosities at higher centre-of-mass energies. On the contrary, the C A,V ϕq and C R uZ,A operator coefficients are more efficiently constrained at centre-of-mass energies ranging approximately between 390 and 550 GeV. At very high energies, the C R,I uZ,A curves saturate to constant values. Individual limits on two-fermion operators are only slightly better for a mostly left-handed polarized beam than for a mostly right-handed polarization (respectively by factors of about 1.03, 1.15, 1.33 for C R,I uA , C A ϕq , C V ϕq and C R,I uZ , relatively independently of the centre-of-mass energy).
The covariance matrix between the measurements of these statistically optimal observables is the inverse of the one which applies on the {C i } extractions and is thus given by Individual one-sigma limits stat. optimal obs.
Individual one-sigma limits stat. optimal obs.  Figure 17. Correlations between the statistically optimal observables measured at a centre-ofmass energy of 380 GeV, for P (e + , e − ) = (0, −80%) and (0, +80%) beam polarizations, respectively below and above the main diagonal. Although they are presented together, note the observable definitions depend on the beam energy and polarization.
Ld ij . For illustration, we display the associated correlation matrices obtained for a centreof-mass energy of 380 GeV and P (e + , e − ) = (0, ∓80%) polarizations in Fig. 17. The cases of left-and right-handed electron beams are respectively shown below and above the main diagonal. Note that the definitions of the statistically optimal observables depend on the centre-of-mass energy and polarization. So, although they are presented together, the sets corresponding to left-and right-handed electron beams are not identical. These correlation matrices clearly indicate that the optimal observables measured in one single run are not independent. Three highly correlated blocs are clearly visible. First, the CP-odd observables relative to the C I uZ and C I uA operator coefficients are basically uncorrelated with all others. The bloc of axial vector operators also stands out from the one formed by vector and dipole operators. To derive constraints in all ten directions of the effective-field-theory parameter space, at least two runs are required with different centre-of-mass energies.
Theoretical robustness We briefly examine the robustness of the statistically optimal observables defined from analytical leading-order amplitudes for the resonant e + e − → tt → bW +b W − process against non-resonant contributions and next-to-leading-order corrections in QCD. Note however that including non-resonant contribution in their definition could be feasible in the future and could enhance the sensitivity to operators affecting top-quark charged currents (as discussed in Sec. 4.4). A proper definition of optimal observables beyond leading order is more involved. To assess their theoretical robustness, we evaluate the optimal observables on a standard-model sample produced for 500 GeV centre-of-mass energy with P (e + , e − ) = (+30%, −80%) beam polarization using MG5_aMC@NLO [21] which implements the complex-mass scheme for the next-to-leading order computation including non-resonant contributions. The corresponding distributions are shown in Fig. 18. The corrections induced onŌ i by non-resonant and NLO contributions are dominated by their effects on the total rate, which are respectively of about 6 and 24%. Residual differences due to shapes are below the couple of percent level except for the observablesŌ A lq ,Ō A eq ,Ō A ϕq associated with axial-vector operator coefficients for which they can exceed ten percent. The non-resonant shape effects can naturally be reduced by cuts on both bW invariant masses. Selecting a 60 GeV window around the top mass for instance bring them below the couple of percent. After this cut, NLO QCD shape corrections on these axial-vector observables can still reach about ten percent. It is to be noted that the top and anti-top reconstruction from the W and b-jet (anti-k t , R = 0.4) of appropriate charge misses a sizeable fraction of the radiation emitted in top-quark decay at NLO in QCD. The reconstructed top and top-anti-top invariant masses notably develop tails towards low values. More sophisticated reconstruction techniques could be imagined. No obstacle however seems to bar the route towards theoretically reliable predictions for the statistically optimal observables of simpler definitions, like the ones used in this work. Although predictions can be much more precise, the observable optimization is then only accurate to leading order. This should be sufficient for all effective-field-theory parameters whose sensitivity mostly arise at that order. We present, in this section, the global reach of top-quark pair production measurements at future lepton colliders. Three benchmark scenarios are considered: circular-collider (CC)-like, ILC-like and CLIC-like. When available, we use the realistic statistical precisions estimated by the corresponding experimental collaborations. To establish a point of comparison, we first present the reach of cross section and forward-backward asymmetry measurements in the ILC-like scenario. The constraints obtained with statistically optimal observables are then presented. The ten-dimensional parameter space that is accessible in top-quark pair production through interferences with SM amplitudes in the vanishing m b limit is considered. The global one-sigma reach is shown, for the three benchmark run scenarios, in Figs. 23, 24 and 25 which constitute our main results. The impact of centre-of-mass energy lever arm and beam polarization is then further examined. An extension of the optimal observable capturing the quadratic dependence of scalar and tensor four-fermion operators is performed in Appendix D.

Uncertainty estimates
We summarize here the assumptions and procedures employed to estimate the precision of top-quark pair production measurements at future lepton colliders. The global reach is rather sensitive to the operating scenario, especially to the centre-of-mass range covered by the machine and to the polarization of the electron and positron beams. We adopt the following benchmark scenarios: CC-like scenario As suggested in Ref. [25], we consider the possibility that a circular lepton collider (CC, for short) would collect 200 fb −1 and 1.5 ab −1 at centre-of-mass of 350 and 365 GeV respectively, without beam polarization. A specific discussion of this scenario is postponed to Sec. 6.5 where the impact of run parameters is examined.

ILC-like scenario
Basing ourselves on Ref. [69], we envisages, in an ILC-like run scenario, the collection of an integrated luminosity of 500 fb −1 at a centre-of-mass energy of 500 GeV and of 1 ab −1 at √ s = 1 TeV. The luminosity is shared equally between the mostly left-handed P (e + , e − ) = (+30%, −80%) and mostly right-handed (−30%, +80%) beam polarization configurations. Compared to Ref. [69], we have modified the scenario in two ways. We ignore the possibility (discussed in Sec. 4.6 and Appendix D) of colliding electron and positron of like-sign helicities. We also give priority to a 1 TeV run over a luminosity upgrade, which could enhance the integrated luminosity at √ s = 500 GeV to 4 ab −1 .   Table 5. Summary of the efficiencies obtained in Refs. [1,19] (first row) and effective rate fractions available for analysis used in this study (second row). When multiplied by the e + e − → tt cross section for the nominal centre-of-mass energy and the integrated luminosity, these yield the number of events available for analysis.

CLIC-like scenario
For estimating measurement uncertainties, we rely on the available full-simulation studies performed by the ILC and CLIC collaborations for the lepton-plus-jets final state obtained after one hadronic and one semi-leptonic top-quark decay [1,19,47]. The charged lepton is taken to be either an electron or a muon. It allows to efficiently tag top and antitop quarks, which is key to an accurate reconstruction of observables such as the forwardbackward asymmetry. Observables such as the top-quark polarization asymmetries are most efficiently reconstructed in this final state. This restriction renders our prospects conservative. The inclusion of the tau-plus-jets and fully hadronic channels is expected to improve the limits significantly, once tau-tagging and jet-charge techniques are fully deployed [68].
Experimental effects affecting the selection and reconstruction of top quark pairs have been identified in the studies referred to above. The most important ones are: − inefficiencies and biases in the selection of lepton-plus-jets events, − migrations due to the finite resolution and incorrect pairing of the top-quark decay products, − losses due to the presence of significant tails in the luminosity spectrum, − uncertainties associated with the subtraction of background processes, notably of single top-quark production at high energies. We base our analysis for the low centre-of-mass energy runs (350 to 500 GeV) on the experimental strategy developed in Refs. [1,47] to address the challenging migrations due to the reconstruction combinatorics. For the high-energy runs, we follow the performance estimates of techniques specifically developed for boosted top-quark reconstruction in Refs. [19,72]. In this case, the luminosity spectrum and the single-top production background are the main limiting factors.
As inputs to the global fits, we use realistic estimates of the expected statistical uncertainties on all observables. Average acceptances times efficiencies are listed in Table 5. For CLIC centre-of-mass energies, they are taken from Ref. [19]. The range of values indicates the difference between the two polarization configurations. The efficiency is typically higher for right-handed electron beam polarizations. For operation at √ s = 380 GeV and 500 GeV the selection efficiency before quality cut is quoted. With a left-handed electron beam, migrations due to poorly reconstructed top-quark candidates are rather pronounced. After eliminating this effect with a stringent quality cut, the acceptance times efficiency for the configuration with a left-handed electron beam is less than 40%.   Figure 19. Global one-sigma constraints and correlation matrix (rounded to the first decimal place) arising from the measurement of cross sections and forward-backward asymmetries in the ILC-like run scenario described in Sec. 6.1 and with the effective tt reconstruction efficiencies given in Table 5 We also calculate the equivalent fractions of the theoretical e + e − → tt rate that is available for analysis, after accounting for efficiency, acceptance, branching ratios and the effect of the luminosity spectrum. Equivalent fractions are averaged for the two polarization configurations and rounded to the next integer. These numbers, presented in the final row of Table 5, are used to determine the statistical uncertainty affecting observable measurements in the following sections.
Systematic uncertainties have been evaluated to some extent in Refs. [1,47]. It is plausible that theoretical and experimental systematics can be controlled to the level of the statistical uncertainties assumed here. We therefore ignore them in the following.
Note that modified optimal observables could be designed to circumvent the reconstruction hurdles mentioned above, symmetrizing their definitions over the two b jets, including single top-quark production contributions in their definitions, or the total invariant mass as additional kinematic variable instead of fixing it to the nominal centre-of-mass energy. We leave such explorations to future work.

Cross section and forward-backward asymmetry
For the sake of comparison with statistically optimal observables, we present in this section the global reach deriving from the measurements of cross sections and forward-backward asymmetries for our ILC-like benchmark scenario. Corresponding results for our CLIC-like scenario are given in Appendix B.
The eight measurements of cross sections and forward-backward asymmetries for two beam polarizations at two centre-of-mass energies are exactly sufficient to constrain the eight CP-conserving operator coefficients which appear at the linear level in these observables. Blue bars in Fig. 19 cover the one-sigma allowed ranges for each of those parameters after marginalization over all others. Numerical values are provided in blue. The assostringent cut is needed for some observables for the run with left-handed electron beam polarization, which reduces the efficiency to approximately 40%.  Figure 20. Eigenvalues and eigenvectors resulting from the diagonalization of the covariance matrix of the global one-sigma constraints deriving from the measurement of cross sections and forward-backward asymmetries (left), or statistically optimal observables (right). In the ILC-like run benchmark scenario described in Sec. 6.1.
ciated covariance matrix is also displayed. White marks indicate individual constraints obtained under the unrealistic assumption that all but the one operator coefficient considered vanish. Numbers for the ratios of marginalized over individual constraints are given in grey. Marginalized constraints are in some cases almost two orders of magnitude looser than individual ones. The constraints on many operator coefficients also appear highly correlated with each other.

Statistically optimal observables
Statistically optimal observables defined on the fully differential bW +b W − final state are linearly sensitive to two CP-violating effective-field-theory parameters in addition to the eight CP-conserving ones accessible with cross section and forward-backward asymmetry measurements (again at the linear level, in the vanishing m b limit). Global constraints for our ILC-like scenario are displayed in Fig. 24. Although the individual sensitivities are not much improved, the use of statistically optimal observables reduces approximate degeneracies in the multidimensional parameter space and therefore also the correlations between global constraints in specific directions. Global limits are then at most a factor of 4 worse than the individual ones. A convenient metric to globally quantify the strength of the constraints in the n-dimensional parameter space of effective-operator coefficient is the so-called global determinant parameter defined as the 2n root of the Gaussian covariance matrix determinant [73]: It evaluates to the geometric average of the semi axes of the one-sigma ellipsoid of constraints. Interestingly, ratios of such quantities are independent of the operator basis used to capture departure from the standard model. Indeed, they are invariant under rotations and rescalings in the space of operator coefficients. This measure is quoted for the eightdimensional parameter space formed by CP-conserving effective-field-theory parameters in both Fig. 19 and Fig. 24. An improvement of by a factor of 1.6 is obtained with statistically optimal observables. This is equivalent to a factor of 2.5 increase in integrated luminosity at both √ s = 500 GeV and 1 TeV (given a 1/ √ L scaling of the GDP).  Profiled chi-squared for each of ten effective operator coefficients constrained through the measurement of statistically optimal observables in the ILC-like benchmark run scenario. Note an unreasonably large vertical axis scale was used to make the difference between the linearised (dashed) and quadratic (solid) effective field theories.
Diagonalizing the covariance matrix reveals the linear combinations of operator coefficients that are least and most tightly constrained. The result is shown for the fit based on optimal observables in Fig. 20 (right) and for the fit relying on the cross section and forward-backward asymmetries in Fig. 20 (left). A linear combination of C V ϕq and C R uZ operator coefficients is least constrained in the two cases. It is also in that direction that the improvement brought by statistically optimal observables is the most significant (more than an order of magnitude). Although the numerical constraints depend on the (arbitrary) operator normalization, the loose bound obtained in that direction when employing cross section and forward-backward asymmetry measurements may lie beyond the range of validity of the linear effective-field-theory approximation. This is explicitly verified by temporarily including quadratic effective-field-theory dependences. The profiled chi-squared for each of the operator coefficients are displayed in Figs. 21 and 22, respectively for cross section plus forward-backward asymmetry and statistically optimal observable measurements. The dashed orange lines are obtained in the linear effective-field-theory approximation. Solid blue lines also include quadratic contributions from dimension-six operators, after expansion of the production, decay, and total width dependences. Note the unreasonably large y-axis scale in Fig. 22. As seen in Fig. 21, the quadratic dimension-six operator contributions significantly affect the constraints obtained with cross section and forward-backward asymmetry measurements. Secondary minima develop in the profiled chi-squared for values of the operator coefficients sometimes far away from what would be allowed in the linear effective-field-theory approximation. This situation is very much improved by the use of statistically optimal observables where quadratic contribution become completely negligible. Results obtained are thus cleaner from the effective-field-theory expansion point of view and can readily be translated from one basis of dimension-six operators to the other.

Global reach
We present, in this section, the global reach offered by statistically optimal observable measurements in the CC-, ILC-and CLIC-like programmes specified in Sec. 6.1 with the overall tt reconstruction efficiencies quoted in Table 5.
As seen in Figs. 23, 24 and 25, individual constraints on C V ϕq and C A ϕq operator coefficients are comparable in all three scenarios. The sensitivity to these operators does not grow with energy and arises mostly at low centre-of-mass energies where the top-quark pair production cross section is maximal. They are more efficiently constrained around √ s 400 and 550 GeV, as seen in Fig. 16. The limits on these vertex operators and on four-fermion operators of identical Lorentz structures are however correlated. Beam polarization or angular distributions are unable to disentangle these two types of contributions. Only runs at different energies can. These correlations are therefore reduced in the ILC-like and, even further, in the CLIC-like scenario. Global constraints come close to individual ones in these cases. The best individual limits on C V ϕq and C A ϕq are obtained in the ILC-like scenario which features the highest degree of polarisation and runs closest to ideal energies. The CLIC-like scenario however provides slightly stronger global constraints thanks to reduced correlations with four-fermion operators. The impact of the centre-of-mass energy   Entries of the covariance matrix are rounded to the first decimal place. Λ = 1 TeV is assumed. The overall tt reconstruction efficiencies quoted in Table 5 are employed at the different centre-of-mass energies. lever arm will be further examined in the following subsection. Individual constraints on vertex operators are one to two orders of magnitude stronger than present ones and at least a factor of three better than the most optimistic HL-LHC prospects, as will be discussed in Sec. 7.1. Global constraints are not available for comparison with the ones we derived for future lepton colliders. This is mostly due to limited sensitivities and more involved analyses at hadron colliders.
Similar observations can be made for the dipole operator coefficients C R uA and C R uZ whose sensitivity only mildly grows with energy (see Fig. 15) but which are still more efficiently constrained at lower centre-of-mass energies (see Fig. 16). Their CP-violating counterparts are, on the contrary, slightly more easy to constrain at higher energies. They are thus somewhat better bounded in ILC-and CLIC-like scenarios. In those two cases, C I uA and C I uZ are also completely uncorrelated with the eight other CP-conserving coefficients. No difference is then observed between their individual and global limits. As will be discussed in Sec. 7.1, present direct individual constraints on CP-conserving dipole operators are two to three orders of magnitude looser than the prospects we obtain at future lepton colliders. The most optimistic HL-LHC reach is still about two orders of magnitude lower. Global constraints comparable to the ones we derive are not available.
Four-fermion operator coefficients benefit greatly from increase in centre-of-mass energy. A clear improvement is therefore seen from CC-to ILC-and CLIC-like scenarios. Four-fermion operators drive the reduction in GDP between ILC-and CLIC-like scenarios, as the constraints obtained on other operator coefficients are similar in these two cases. GDP ratios between CC, ILC and CLIC constraints are 30 : 2.2 : 1. To match CLIC level of constraints, the corresponding overall increase in luminosity required at the ILC and CC are respectively of 4.8 and 990 for all centre-of-mass energies (given our inclusion of statistical uncertainties only, GDPs scale as 1/ √ L). Although a direct comparison between the two-lepton-two-quark operators of interest here and the (colour octet) four-quark operators presently probed in top-quark pair production at the LHC is not strictly speaking possible, CC-like scenario would probes four-fermion operator couplings a factor of a few smaller, and a ILC-or CLIC-like scenarios two to four orders of magnitude smaller (see Sec. 7.2). For comparisons in terms of scales probed for unit couplings, the square root of those factors applies.

Exploring run scenarios
Beside comparing the constraining power of different sets of observables or benchmark scenarios, an interesting exercise one can perform with GDP ratios (see definition in Eq. (6.1)) is to optimize run parameters to set the strongest overall constraints. Note however that different optimizations would be obtained in specific models of new physics privileging certain directions in the effective-field-theory parameter space.
Sharing luminosity A first possibility is to vary the share of integrated luminosity spent with each polarization configuration and at the 500 GeV and 1 TeV centre-of-mass energies It yields a GDP of 0.01471 which scales with the total integrated luminosity as 1/ √ L. This is only a factor 1.005 better than in our benchmark scenario. Variation around this minimum with the fraction of integrated luminosity spent at √ s = 1 TeV and with both polarization configurations are shown in Fig. 26. Adding the possibility of run at √ s = 380 GeV does not lead to any noticeable improvement and the strongest constraints are found for a vanishing fraction of the total integrated luminosity spent at that energy. On the contrary, it requires about 4.6 ab −1 shared between √ s = 380 and 500 GeV runs to achieve the same overall performance. The optimal run parameters are then: √ s = 380 GeV 1.5 ab −1 57% with P (e + , e − ) = (+30%, −80%) 500 GeV 3.1 ab −1 51% .
Equivalently, sharing 1.5 ab −1 between those two lower-energy runs, one would obtain a GDP that is approximately 1.8 times worse.

Reducing beam polarization
The impact on the electron and positron beam polarization can also be studied using GDP ratios. As illustration, we consider again the ILC-like benchmark scenario described earlier with runs at centre-of-mass energies of 500 GeV and 1 TeV and decrease the absolute magnitude of each beam polarization separately. Figure 27 shows the ratio of the obtained GDP with the one obtained with P (e + , e − ) = (±30%, ∓80%). It is seen that the magnitudes of the electron and positron polarizations are equally important. A decrease of 10% in either of them leads to a decrease in GDP of about 5% which could be compensated by an overall 11% increase in luminosity at both centre-of-mass energies. In particular, vanishing positron polarization leads to a degradation of the statistical constraints by a factor of 0.85 and could be compensated by an overall 38% increase in integrated luminosities. The absence of beam polarization degrades the optimal-observable constraints by an average factor of about 2.15 compared to the benchmark scenario. The global constraints on C I uZ are the most affected (degraded by a factor of 8), followed by C V eq , C I uA , C R uZ , C V ϕq and C V lq (degraded, respectively, by factors of 3.5, 2.7, 2.6, 2.5 and 2.5).   Figure 28. Improvement in the GDP brought by an increasing centre-of-mass energy lever arm. Statistically optimal observables are measured in runs at two different energies, with P (e + , e − ) = (0%, ±80%) beam polarizations. Perfect efficiency on the tt reconstruction has been assumed. An overall efficiency of would rescale GDPs by a 1/ √ factor. Note the exact top-quark mass (m t = 172.5 GeV), the leading-order and narrow top-quark width approximations used could affect results obtained near threshold.
Reference [15] stressed that the measurement of observables that are sensitive to the top-quark polarization can compensate for the lack of beam polarization. We indeed find that the observables studied in Sec. 4.2 have good sensitivity to effective operator coefficients and provide complementary information. The analysis of statistically optimal observables nevertheless shows that operation with two beam polarizations provides an important improvement of the results.
Impact of the energy lever arm Runs at two separate centre-of-mass energies are indispensable to distinguish two-and four-fermion operators. Figure 28 shows that the average constraint strength -in terms of GDP-brought by the measurement of statistically optimal observables decreases significantly with the separation between available centre-of-mass energies. Three scenarios are displayed. The first one (blue curve) includes 100 fb −1 gathered at √ s = 350 GeV and 500 fb −1 at a higher energy point. A dramatic increase is brought by the first few tens of GeV of lever arm. A second scenario includes runs at 350 and 380 GeV in addition to x fb −1 collected at a higher x GeV centreof-mass energy. A third scenario also includes a fixed 1.5 ab −1 gathered at 1.4 TeV. Two P (e + , e − ) = (0%, ±80%) beam polarizations and perfect tt reconstruction efficiencies are assumed.
Compared to our benchmark ILC-like scenario, combining runs at 380 and 500 GeV with 500 fb −1 equally shared between P (e + , e − ) = (±30%, ∓80%) polarizations at both energies would degrade the GDP by a factor of 2.0. Equal overall statistical performances would require 4.0 times higher luminosities at both 380 and 500 GeV. The four-fermion operators are the most affected, with global constraints about five and seven time worse for vector and axial-vector ones. The least affected are C V ϕq and C R uZ constraints with a degradation by factors of about 1.2.

Circular collider scenario
Degrading the polarization magnitude and centre-of-mass energy lever arm to the extreme, one obtains conditions that future circular colliders will be facing for tackling top-quark physics. As mentioned earlier, they could perform runs at the top-quark pair production threshold and, only few GeV higher, at 365 GeV, without beam polarization. The global constraints deriving from the measurements of statistically optimal observables are displayed in Fig. 23 and were already somewhat discussed in the previous subsection. They are significantly looser than that achievable with linear colliders, with GDPs respectively 14 and 31 times worse than in ILC-and CLIC-like scenarios. Correlations and the ratios of global to individual constraints are also large. One could therefore expect the linear effective-field-theory approximation to break down. Figure 29 however seems to indicate that quadratic contributions still have a limited impact on onesigma constraints.
Introducing P (e + , e − ) = (±30%, ∓80%) beam polarizations and sharing the same amount of integrated luminosity equally among them improves the GDP by a factor of two. Global constraints on the C I uZ , C V ϕq , C V eq , C I uA and C V lq coefficients benefit from the strongest improvements with factors of 9.6, 3.6, 3.2, 3.2 and 2.8 respectively. The strengthening of individual constraints is less significant, indicating that beam polarization mostly helps lifting approximate degeneracies instead of improving sensitivities. When Figure 29. Profiled chi-squared deriving from the measurements of statistically optimal observables for a circular collider (CC-)like run scenario with the overall tt reconstruction efficiencies quoted in Table 5. Solid blue lines include quadratic effective-field-theory dependences while dashed orange ones are obtained in the linear approximation.
exploiting the pair-production threshold region for coupling measurements, it is worth keeping in mind it is usually primarily employed to determine precisely the top-quark mass and width, assuming couplings are sufficiently constrained by runs at higher energies. To our knowledge, no study of the threshold region has so far included top-quark effectivefield-theory dependences and analysed their impact on mass and width determinations.

Comparison with existing limits and HL-LHC prospects
In this section, lepton-colliders prospects are compared to existing limits on the top-quark effective field theory arising from fit to Tevatron and LHC data. The indirect limits deriving from low-energy measurements are briefly discussed. Prospects for the remaining of the LHC programme are also examined.

Hadron-collider sensitivity to two-fermion operators
The Tevatron and LHC experiments are sensitive to top-quark electroweak couplings through several measurements. Charged-current interactions of the top quark are sensitive to several of the operators studied in this paper. The tbW vertex has been characterized thoroughly in studies of top-quark decay and is also probed in the electroweak single-top production processes at hadron colliders.
Existing constraints ATLAS and CMS published measurements of the longitudinal and left-and right-handed helicity fractions F 0 , F L and F R of the W boson in top-quark decays [77,78] having a precision of 2 to 3%. The rate of single top-quark production in the t-channel, first observed at the Tevatron [79,80], is precisely measured at the LHC, with errors on the fiducial cross section ranging from 6 to 8% [81,82]. Single top-quark production in the s-channel was so far only observed at the Tevatron [83]. Reference [74] combined the measurements of the single top production cross sections and the W helicity fractions in top-quark decay at √ s = 8 TeV in an analysis involving existing expected at high luminosity expected at e + e − TopFitter Ref. [74] Ref. [74] ttV [14,75] Table 6. Individual 95% C.L. limits on two-quark operator coefficients deriving from measurements at hadron colliders. The first two columns show the existing limits derived by the TopFitter group [59] and in Ref. [74]. The next four columns are expected limits with 3 ab −1 of integrated luminosity at the LHC, derived from single top and top decay measurements [74], from differential distributions in ttV production [14,75], and from the total ttV cross sections measured with 10% and 3% precision. The tZj columns show limits expected with 300 fb −1 using a p T (t) > 250 GeV selection cut. The last three columns are the individual limits obtained in this work for CC-, ILCand CLIC-like run scenarios. As discussed in Sec. 6.4 individual constraints are similar in those three cases although global ones are less so.
only the three anomalous couplings affecting the tbW vertex. These constraints can be converted 8 to the 95% C.L. limits on the effective operator coefficients displayed in the second column of Table 6, for Λ = 1 TeV. Dedicated measurements of angular distributions and asymmetries in single top-quark production can provide slightly more stringent limits than the inclusive cross section measurement [84][85][86].
More recently, the Tevatron and LHC have gained access to associated production processes, where a top-quark pair or single top quark is produced together with a photon [87][88][89][90] or Z boson [91][92][93][94]. Measurements of the production rates yield limits on the ttγ and ttZ vertices. The existence of these processes is now firmly established, but the precision of the rate measurements is still quite limited: the inclusive production cross sections are currently known to 20 − 30% precision.
Single top-quark production in association with a Z boson probes both the charged current interactions (when the Z boson is produced through W fusion) and the interactions with the Z boson (when the Z boson is radiated off the top quark). This process has been observed in LHC run II and cross-section measurements at √ s = 13 TeV by ATLAS [93] and CMS [94] are in good agreement with standard-model predictions within an experimental uncertainty of approximately 30%. At this level of accuracy, the limits on relevant dimension-six operators are not competitive with respect to other processes such as ttV and single top-quark production. Evidence for single top-quark production in association with a photon has also been found very recently by the CMS collaboration [90]. The associated cross section measurement has an uncertainty of about 40%.
The most complete effective-field-theory analysis of the top-quark sector to date was performed by the TopFitter group. It took into account a large collection of Tevatron 8 The fit of Ref.   Figure 30. Summary of 68% C.L. limits on the C V ϕq and C A ϕq coefficients of the two-fermion operators that affect the left-and right-handed couplings of the top quark to the Z boson and the dipole operators C R uA and C R uZ . Individual limits from Tevatron plus LHC run I data are taken from Ref. [59] and are converted to the conventions we use by assuming Gaussian probability distributions and by neglecting the unpublished correlations. For the ILC-and CLIC-like scenarios, individual and global constraints are presented. The conversion between our conventions and that of the LHC TOP WG [26] are detailed in Appendix E. and LHC run I measurements [17,59,95], performing a global analysis including nine operator coefficients. Individual constraints were derived on three others. The conversion of these limits to our normalization is provided in Appendix F.
We present in Table 6 a summary of the individual limits derived from the Tevatron and LHC data by the TopFitter group [59] and in Ref. [74]. For comparison, prospects obtained in this paper for the CC-, ILC-and CLIC-like run scenarios are given in the last three columns of the same table. The existing individual constraints obtained by the TopFitter group are visually compared to ILC and CLIC prospects for two-fermion operators in Fig. 30. For this figure, the rotation to our basis of operator coefficients is performed by assuming the unpublished correlations between TopFitter limits vanish. Any of the three e + e − collider scenarios considered improves the individual limits by over an order of magnitude.
Prospects Several authors have studied the expected evolution of LHC limits during run II and III as well as after its high-luminosity phase. Reference [74] presented limits expected from helicity fractions and single top-quark cross section measurements (the latter based partially on Ref. [96]) after the complete LHC programme (3 ab −1 at √ s = 14 TeV) that are only marginally stronger than the existing ones.
Several studies of the prospects for the determination of the top-quark couplings to the photon and Z boson have been performed. Reference [17] estimated that constraints arising from inclusive σ(pp → ttZ) measurements would improve by at most a factor of two with the high-luminosity phase of the LHC. The precision of the SM prediction, approximately 10% at NLO, may limit the progress of the constraints derived from the inclusive cross section. Reference [97] considered the construction of two ratios of cross sections R Z,γ = σ ttZ,γ /σ tt which can be predicted with a precision of 3% and thus avoid this limitation. An analysis of differential cross sections may also enhance the sensitivity. References [14,75] derived better limits for 3 ab −1 collected at 13 TeV by considering the p T distribution of the Z boson and the ∆φ ll angular distribution of the leptons arising from the Z-boson decay.
We estimate individual 68% C.L. limits on four operator coefficients under several assumptions for the precision of the inclusive pp → ttV cross section measurement at the LHC. The dependence of the cross section on the coefficients is taken from Ref. [20] for the first three operators, up to quadratic order, and estimated in a similar fashion for C uB . The first scenario considers a precision of 30%, which corresponds roughly to the first measurements at the LHC. The limits we obtain are indeed similar to those of the TopFitter group. The second scenarios envisages a precision of 10%, which matches the approximate theoretical uncertainty of current next-to-leading order calculations. The third scenario, with 3% precision, represents the ultimate precision envisaged in Ref. [97]. The projections for the latter two scenarios are displayed in the fifth and sixth columns of Table 6.
With a large integrated luminosity tZ production allows to access higher-p T regions, where the sensitivity to dimension-six operators is enhanced by the breaking of standardmodel unitarity cancellations they induce. In Ref. [76], this effect is studied and projections are derived for 300 fb −1 of integrated luminosity. These results are displayed in the seventh column of Table 6.
The improvement during the remaining LHC program and its high-luminosity stage is quite substantial for all two-fermion operators, primarily driven by precision measurements of rare associated production processes. The limits on C 1 ϕq , C 3 ϕq and C ϕu may improve by nearly an order of magnitude in the most optimistic scenario. Improvements are milder for the dipole operators C uB and C uW -by a factor of three-as for these operators the quadratic term is dominant.
An energy upgrade of the LHC in the existing tunnel [98] or a new 100 TeV pp collider [99,100] would dramatically increase the sample size for top-quark associated production processes and thus present important opportunities for precision measurements of their rates [101]. The dependence of the inclusive cross section on the dimension-six operator coefficients grows only very slowly with increasing centre-of-mass energy, but differential measurements in the transverse momentum of the Z-boson or photon can strongly enhance the sensitivity [75]. A detailed evaluation of the potential for measurements of the electroweak couplings of the top quark remains to be performed.
We conclude that electron-positron colliders offer excellent potential to probe new physics through the two-fermion operators considered in this section, even at a relatively modest centre-of-mass energy, between 350 and 500 GeV. Comparison of the expected individual limits for the CC-, ILC-and CLIC-like scenarios with the projections for hadron colliders 95% C.L. limits from Tevatron + LHC run I C 1  Table 7. 95% C.L. limits on four-fermion operators obtained in a nine-parameter fit of top physics measurements at the Tevatron and LHC run I. The results are presented without the factor v 2 /Λ 2 that Ref. [59] applies.
shows that the sensitivity of e + e − machines exceeds that of the Tevatron and LHC run I by one to three orders of magnitude. Improvements of the limits during future LHC runs and its high-luminosity phase are limited to factors 1.5 to 25, in the most optimistic scenario.
A linear e + e − collider therefore seems the most promising project to reach the ultimate precision in the determination of two-fermion operator coefficients that affect top-quark electroweak couplings.

Hadron collider sensitivity to four-fermion operators
In this section, we compare the limits on the coefficients of the e + e + tt operators studied in this paper with limits that can be set on the coefficients of qqtt operators at hadron colliders. As these two sets of operators are of different nature, the conclusion of such an exercise must be interpreted with caution. 9 Existing constraints Unpolarized top-quark pair production at hadron colliders is only linearly sensitive to four combinations of qqtt operator coefficients, denoted [36]. The C 1 q + C 2 q sums and C 1 q − C 2 q differences respectively appear in the total cross section and production asymmetry (A FB at the Tevatron, or A C at the LHC [102]). The individual and global nine-parameter 95% C.L. limits obtained from Tevatron and LHC run I data in Ref. [59] are reproduced in Table 7. They take into account the measurements of asymmetries, as well as inclusive and differential cross-sections. 10 The global limits range from |C| 2.5 to |C| 9. For couplings of order one, these correspond to new-physics scales between 300 to 600 GeV. The limits on C u 1 and C d 1 are a factor two to three better than limits on C u 2 and C d 2 . Individual limits are a factor two to five stronger than the results of a global fit.
The global limits on four-fermion operators from the ILC-like scenario are of order 2 × 10 −3 . The limits in the CLIC-like scenario, with the powerful constraint from operation at √ s = 3 TeV, are of order 3 × 10 −4 . For couplings of order one, these correspond to scales between 20 and 60 TeV. 9 The four-fermion operators affecting e + e − → tt production can in principle be probed at hadron colliders, in pp → tte + e − production, but the sensitivity is likely limited and no such analysis has been performed so far. 10 In the conventions of the LHC TOP WG [26], the definitions of Ref. [59] correspond to C 1 Qq . Note that C 1 d originally defined in Ref. [36] is a factor of four larger.

Prospects
The LHC limits are expected to improve as run II and III accumulate a larger sample. As inclusive cross-section and charge asymmetry measurements are limited by systematic uncertainties, most of the gain is expected to come from the boosted regime, where the sensitivity to four-fermion operators strongly grows. After run I, the cross section and charge asymmetry measurements in the boosted regime yield limits of strength comparable to those deriving from inclusive measurements [103,104]. As the integrated luminosity of the data set at √ s = 13 TeV increases, such measurements can drive a steady progress of the constraints. An order of magnitude improvement of the limits is within reach, provided that the measurements in the boosted regime (m tt > 1 to 1.5 TeV) achieve a precision similar to the inclusive measurements in run I [104].
With 300 fb −1 , four-top production can provide competitive constraints on the qqtt operators, in models for which contributions due to powers of dimension-six operator coefficients as high as four are dominant with respect to that of higher dimensional operators [105]. With 3 ab −1 , the estimated precision on the total four-top production cross section improves by a factor of about two. Limits on operator coefficients are however only strengthened by the fourth root of this factor.
The potential of hadron colliders reaching even higher energies remains to be explored. Reasonably precise measurements of the tt production cross section and charge asymmetry in an extremely boosted regime, with m tt > 10 TeV, seem feasible [106]. The sensitivity of such measurements to qqtt operators increases by two orders of magnitude.
We conclude that the projected bounds on the coefficients of e + e − tt operators in ILCand CLIC-like run scenarios are approximately four orders of magnitude more stringent that the current bounds on the C 1 u , C 2 u , C 1 d , C 2 d coefficients of colour-octet qqtt operators. This represents a gain of about two orders of magnitude in terms of the scale that is probed, for identical couplings. While very naive, this comparison shows rather eloquently how the precision of the measurements in an e + e − collider allows to probe high energy scales, compensating for the relatively low direct energy reach.

Indirect limits
Indirect limits on top-quark operators can be derived using the renormalization group (RG) running and mixing of operator coefficients. These arise from loop contributions that are enhanced by logarithmic log Λ 2 terms. They are however indirect because tree level contributions (into which the top-quark operators mix) are always present. Whether they can be safely neglected depends on the model. RG-induced limits have been derived on a number of operators in Ref. [107]. The RG evolution of the entire group of dimension-six operators was used to estimate the impact of operators involving top quarks on electroweak precision measurements at LEP and SLD. Λ 2 ). The individual limits on C 1 ϕq , C 3 ϕq and C ϕu are of the order of 0.05. A two-parameter fit yields marginalized limits that are 5 to 10 times looser.
Electroweak precision observables, namely δg b L and the T parameter, are considered in Ref. [109] together with the K + → π + νν and B s → µ + µ − rare meson decays. The authors assume C 1 ϕq + C 3 ϕq = 0 to satisfy the Z → bb constraints at LEP. The loop-level contributions from C 3 ϕq and C ϕu are proportional to log µ W /Λ, where µ W is the electroweak scale. The coefficients C 3 can be constrained to the order of a few percent, which translates to about 0.5 on C 3 ϕq and C ϕu assuming Λ = 1 TeV. The above limits are based on strong assumptions, namely that only one operator receives a non-zero initial condition at the scale Λ. In particular, tree-level contributions from other operators into which the top-quark operators mix are set to zero. To obtain more reliable limits, one should include the finite (i.e. non-logarithmic) term from the loop contribution. This allows limits to be extracted by marginalising over the tree level contributions. For example, a global fit to all electroweak precision observables was performed in Ref. [110], including loop contributions from dimension-six top-quark operators, and marginalising over the O ϕW B and O ϕD operators, which are often identified as the S and T parameters. The resulting limits are scale-independent, in contrast to the RG-induced ones. The individual 68% C.L. constraints are: Finally, at the LHC, top-quark operators enter Higgs boson production and decay processes through top-and bottom-quark loops. Higgs signal strength measurements thus constrain top-quark operators indirectly. The corresponding limits were derived in Ref. [111] using projected Higgs measurements at the LHC, with 3 ab −1 , including differential distributions. The resulting 95% C.L. individual limits on the relevant operators in this work are: These are based on the assumption that other Higgs operators do not modify the Higgs signal strengths. However the EFT scale is set to m H . Therefore, the log-enhanced terms are not used and the results can be considered as an estimate of the indirect sensitivity at the high-luminosity LHC. Also note that marginalised bounds are much weaker.
Almost all individual indirect limits presented in this section are much stronger than the existing bounds deriving from LHC and Tevatron measurements and shown in Table 6. They however rely on model-dependent assumptions. Nevertheless, they are still weaker than direct limits expected from linear colliders, by about one order of magnitude. Therefore, our conclusion that a linear collider is the most promising project for determining top-quark electroweak couplings holds even in comparison with these indirect bounds.

Conclusions
We evaluated the potential of future lepton colliders to reveal new physics effects in precision measurements of top-quark pair production. A broad set of dimension-six operators was considered, affecting notably the electroweak interactions of the top quark. Fourfermion e + e − tt operators and the CP-violating imaginary parts of electroweak dipole operators were also included. Predictions at next-to-leading order in QCD for these operators were made available in the MG5_aMC@NLO framework.
We studied the sensitivity of a large number of observables, as well as the impact of the centre-of-mass energy and beam polarization. Combining measurements of the top-quark polarization and of CP-odd observables with that of the cross section and forward-backward asymmetry increases the sensitivity to the real and imaginary parts of the dipole operators, respectively. We also examined the power of additional constraints, such as the measurement of the top-quark width in a threshold scan or of bottom-quark pair production. We observed that even with an extended set of observables, control over the beam polarization remains an important handle to simultaneously constrain the contributions of vector and axial-vector operators. Operation at high centre-of-mass energy provides tight bounds on four-fermion operators whose contributions grows quadratically with the energy, with respect to standard-model ones. The inclusion of data acquired at two centre-of-mass energies is crucial in a global fit of two-fermion and four-fermion operators.
To effectively and simultaneously cover all considered directions of the effective-fieldtheory parameter space, we constructed a set of statistically optimal observables that maximally exploits the information contained in the fully differential bW +b W − distribution. The global reach achieved with their measurements considerably exceeds the one obtained through the determination of cross sections and forward-backward asymmetries only. A combination of statistically optimal observable measurements at two different centre-ofmass energies is sufficient to simultaneously constrain the ten operator coefficients considered. Larger separations between the two centre-of-mass energies resolve approximate degeneracies and bring global limits closer to individual ones. Beam polarization helps increasing individual sensitivities and reducing global correlations.
Our study takes into account experimental effects in the selection of lepton-plus-jets events, the reconstruction of the top-quark candidates, the presence of background processes and of significant tails in the luminosity spectrum. We use conservative estimates for the effective efficiency needed to reproduce the statistical uncertainties obtained in fulldetector simulation studies. It is expected that systematic uncertainties can be controlled to a similar level.
Improved statistically optimal observables could help addressing identified reconstruction challenges in the future. Definitions symmetrized over the two final-state b jets could mitigate the impact of migrations due to the mis-pairing of top-quark decay products that are important at low energies, especially with a left-handed electron beam polarizations. In an inclusive e + e − → bW +b W − analysis, accounting for the effective-field-theory dependence of non-resonant contributions would effectively turn the single top-quark production background which becomes large at high energies into a signal component. Considering the centre-of-mass energy as an additional kinematic variable instead of fixing it to its nominal value in the optimal observable definitions could also help exploiting the significant lower tail of the beam-energy spectrum which develops in TeV operation.
The projected reach of circular-collider-, ILC-and CLIC-like operation scenarios was presented in Figs. 23, 24 and 25, respectively. The individual limits on the coefficients of the operators modifying top-quark electroweak couplings are one to three orders of magnitude better than present constraints. Improvements by factors of three to two hundred are also expected compared to the most optimistic prospect for the individual reach of the HL-LHC. Clean global analyses are moreover readily achievable at future lepton colliders, yielding robust direct constraints of limited model dependence.

A Effective-field-theory expressions for anomalous vertices
Anomalous vertices have been widely used to parametrize interactions of the top quark beyond the standard model. Following Ref. [5], the Z, γ → tt and t → bW + vertices can be written as When it exists, the correspondence with the fully gauge invariant effective field theory described in Sec. 3 is given the following: Λ 2 i C I uA = Im{C (33) uW + C (33) uB } , It is however worth stressing a few shortcomings of the anomalous coupling approach. An important one is that it completely misses four-fermion operators which are often generated at tree-level when introducing new heavy states beyond the standard model.
anomalous couplings also break electromagnetic gauge invariance. Their inclusion would thus render the theory sick and preclude the computation of quantum corrections. Finally, the anomalous couplings of the top quark to a photon or Z boson are in general allowed to be complex although they then break unitarity.

B Additional results for the CLIC-like scenario
We provide here additional results corresponding to the CLIC-like benchmark run scenario introduced in Sec. 6.1. The sensitivities of the total and forward-backward-integrated cross sections, as functions of the centre-of-mass energy and for a vanishing positron polarization are shown in Fig. 31. Individual constraints deriving from the measurements of the cross section or forward-backward asymmetry are shown in Fig. 32. They are normalized for an integrated luminosity times efficiency of 1 ab −1 . With the overall tt reconstruction efficiencies of Table 5, the global constraints resulting from the measurements of cross sections and forward-backward asymmetries are displayed in Fig. 33. For C V ϕq and C R uZ , they are almost an order of magnitude looser than the individual constraints. Although we do not study the impact of the quadratic effective-field-theory dependences, it can be expected to be non negligible, as in the ILC-like scenario.
The sensitivities of each statistically optimal observable to the corresponding operator coefficient, as functions of the centre-of-mass energy, are displayed in Fig. 34. The individual constraints deriving from optimal observable measurements, normalized for a 1 ab −1 integrated luminosity times efficiency, are shown in Fig. 35. The global constraints were already presented in Fig. 25, on page 36. The global determinant parameter on the eight-dimensional space of CP-conserving parameters is improved by a factor of about Individual one-sigma limits from cross section Individual one-sigma limits from forward backward asymmetry   Table 5 are assumed and Λ is fixed to 1 TeV.   Figure 34. Sensitivity of each statistically optimal observable to the corresponding operator coefficient, as a function of the centre-of-mass energy, and for P (e + , e − ) = (0%, ±80%) beam polariza- Individual one-sigma limits stat. optimal obs.
Individual one-sigma limits stat. optimal obs. 1.4 compared to the one obtained from the measurements of cross sections and forwardbackward asymmetries. Most importantly, the correlation between operator coefficients is reduced and their global limits approach their individual ones. Sensitivity to the quadratic dependence of the dimension-six operator coefficients is thus expected to be limited, so that clearner effective-field-theory results are obtained.

C Selected results at NLO in QCD
MG5_aMC@NLO [21] is employed with the following input parameters: The TEFT_EW UFO model [20] is extended to include four-fermion operators and imaginary coefficients for the electroweak dipole operators. The necessary UV and R2 counterterms required for simulation at NLO in QCD are implemented. The effective-field-theory dependence of the top-quark width is also taken into account.
The total and forward-backward-integrated cross sections for which we now provide the linear effective field theory dependence at next-to-leading order in QCD are parametrized as follows: The linear σ i dependences are provided in Tables 8 and 9. Central values, k-factors, scale and Monte-Carlo uncertainties will be formatted as central value The scale uncertainty is computed from the running of α S (µ) between µ = m t /2 and 2m t .

D Optimal observables for scalar and tensor four-fermion operators
Some observables sensitive O S,T lequ were already discussed in Sec. 4.6. The set of statistically optimal observables can also be extended to achieve sensitivity to scalar and tensor fourfermion operators. Due to their chirality, these operators do not interfere with standardmodel amplitudes (in the limit of vanishing lepton masses) and yield no linear dependence in the bW +b W − differential distribution. The standard prescription for the construction   of statistically optimal observables can therefore not be applied. One can however still define observables that are optimally sensitive to their quadratic dependences. Because these two operators do not interfere with their own Hermitian conjugates, only dependences on |C S lequ | 2 , |C T lequ | 2 , Re{C S lequ C T * lequ }, and Im{C S lequ C T * lequ } are generated. Four optimal observables corresponding to each of these terms in the e + e − → tt → bW +b W − differential distribution can thus be defined. Three new physical degrees of freedom are introduced, namely two norms and one relative phase. The mapping between these quantities and the optimal observables associated to |C S lequ | 2 , |C T lequ | 2 , Re{C S lequ C T * lequ }, Im{C S lequ C T * lequ } is both non-linear and subject to constraints: norms are positive and the phase has a period of 2π. The additional four statistically optimal observables are still defined at leading order and in the narrow width approximation, on the bW +b W − final state. A numerical method based on amplitudes computed by MG5_aMC@NLO [21] in its standalone c++ mode is used to define them. Unlike the analytical approach used so far, it does not include the subleading effective-field-theory dependence arising in top-quark decays. The good agreement obtained cross-validates the two methods.
A ILC-like benchmark scenario is assumed as before, with runs at centre-of-mass energies of 500 GeV and 1 TeV. The global Gaussian constraints on the set of 14 operator coefficient combinations which include |C S,T lequ | 2 and Re, Im{C S lequ C T * lequ } in addition to the 10 coefficients previously considered are displayed as blue bands in Fig. 36. For comparison, dark blue arrows show the bounds obtained without including scalar and tensor operators. At this stage no relation is assumed between the different quadratic combinations of scalar and tensor four-fermion operators. Expressing them as functions of two norms and one relative phase as well as imposing constraints on the domain of those quantities (norms are positive and phases have a period of 2π) leads to the limits shown as arrows of a lighter shade of blue. The largest absolute value is retained as constraints become non-Gaussian and asymmetric around zero after this non-linear transformation. After marginalization over other degrees of freedom the relative phase between C S lequ and C T lequ is left unconstrained and is therefore not displayed in Fig. 36. By default, all four P (e + , e − ) = (±30%, ±80%) beam polarizations are used. The +− and −+ (++ and −−) polarizations receive each 40% (10%) of the total luminosity at each centre-of-mass energy. Splitting the integrated luminosity equally between the +− and −+ ones, as before, leads to the constraints shown with arrows of the lightest shade of blue.
It is seen that introducing scalar and tensor operators mildly loosen the constraints on other four-fermion operators. Runs with ++ and −− beam polarizations help mitigating this effect and strengthen the constraints on |C S,T lequ | 2 , as expected. The resulting reduction of integrated luminosity spent on +− and −+ beam polarization configurations causes a limited degradation of constraints in some other directions of the effective-field-theory parameter space. Overall, the use of like-sign beam polarizations yields an improvement by a factor of about 1.1, in terms of GDP defined on the Gaussian constraints in the space of 14 combinations of operator coefficients artificially treated as independent degrees of freedom without constraints on their domain.   Figure 36. Global constraints deriving from the measurements of a set of statistically optimal observables extended to include dependences on the scalar and tensor four-fermion operators for a modified ILC-like run scenario. Runs collecting 500 fb −1 at 500 GeV and 1 ab −1 at 1 TeV, as well as the overall tt reconstruction efficiencies of Table 5 are assumed. The four P (e + , e − ) = (±30%, ±80%) beam polarizations are exploited, the +− and −+ (++ and −−) receiving each 40% (10%) of the integrated luminosity.

E Conversion to LHC TOP WG EFT conventions
The effective-field-theory conventions employed in this paper are somewhat different than the standards recently established by the LHC TOP WG in Ref. [26]. We provide here the conversion to those standards: Our main results, the constraints deriving from the measurements of statistically optimal observables are translated to those conventions for the CC-, ILC-and CLIC-like scenarios in Fig. 37. Because these conventions are less natural to the description of the top-quark pair production process at lepton colliders, larger correlations are present. The qualitatively different sensitivities to vector and axial vector operators would not have been manifest either with these degrees of freedom.

F Conversion of TopFitter limits
This appendix details the conversion to our normalizations of the limits obtained by the TopFitter group [17,59,95] on the operator coefficients relevant for top-quark production  Figure 37. Global one-sigma constraints and correlation matrices deriving from the measurements of statistically optimal observables for circular-collider-(top), ILC-(centre) and CLIC-like (bottom) run scenarios, in the effective-field-theory conventions established by the LHC TOP WG [26]. The overall tt reconstruction efficiencies of Table 5 are employed and Λ is fixed to 1 TeV. White marks stand for the individual constraints obtained when all other operator coefficients vanish. Dashed vertical lines provide the average constraint strengths in terms of GDP.
ind. 95% C.L. 68% C.L. present run III or HL ind. 95% C.L. glo. 95% C.L. ind. 95% C.L. glo. 95% C.L.  Table 10. Individual and global constraints derived by the TopFitter group, in the normalization employed in this paper. The results in the first six columns correspond to an analysis of Tevatron and LHC run I measurements. The last four columns the individual and global prospects made in Ref. [17] for the constraints from measurements of the e + e − → tt cross section and forwardbackward asymmetry measurements. We set Λ = 1 TeV. The numerical values for Fig. 7 of Ref. [59] have been obtained from a quartic fit to the likelihood provided by the authors. Others are directly obtained from the figures. at lepton colliders. The conversion factors are the following: where v 246 GeV, y t 0.99, g 0.65 and g 0.35. The individual and global limits obtained in these references are displayed in Table 10. The first five columns correspond to the analysis of Tevatron and LHC run I measurements performed in Ref [17,59]. Prospects for LHC run III or its high-luminosity phase are given in the sixth column. They are extracted from Fig. 2 of Ref. [17]. In its last four columns, Table 10 also presents the individual and global prospects made in Ref. [17] for cross section and forward-backward asymmetry measurements in e + e − → tt production. The measurements are assumed to have total relative uncertainties of 2% for each of the three P (e + , e − ) = (±30%, ∓80%), (0%, 0%) beam polarizations at either √ s = 500 GeV or 3 TeV.