Consistent constraints on the Standard Model Effective Field Theory

We develop the global constraint picture in the (linear) effective field theory generalisation of the Standard Model, incorporating data from detectors that operated at PEP, PETRA, TRISTAN, SpS, Tevatron, SLAC, LEPI and LEP II, as well as low energy precision data. We fit one hundred and three observables. We develop a theory error metric for this effective field theory, which is required when constraints on parameters at leading order in the power counting are to be pushed to the percent level, or beyond, unless the cut off scale is assumed to be large, Λ ≳ 3 TeV. We more consistently incorporate theoretical errors in this work, avoiding this assumption, and as a direct consequence bounds on some leading parameters are relaxed. We show how an S, T analysis is modified by the theory errors we include as an illustrative example.


JHEP02(2016)069 1 Introduction
The linear Standard Model Effective Field Theory (SMEFT) assumes that SU(2) L × U(1) Y is spontaneously broken to U(1) em by the vacuum expectation value of the Higgs field (v) and that the observed 0 + scalar is embedded in the Higgs doublet. It also assumes that the low energy limit of beyond Standard Model physics (BSM) is adequately described when SU(3) × SU(2) L × U(1) Y invariant higher dimensional operators built out of the Standard Model (SM) fields, are added to the renormalizable SM interactions. 1 The Lagrangian is schematically L SMEFT = L SM + L 5 + L 6 + L 7 + · · · (1.1) There is one operator in L 5 , suppressed by one power of the cut off scale(Λ) [2]. In L 6 there are 59 (+ Hermitian conjugate) operators that preserve Baryon number [3,4], and four operators that violate Baryon number [2,5]. L 7 contains thirty operators that all violate lepton number [6,7]. Recently L 8 has been classified [7,8] and counts 993 N f = 1 operators. The discovery of a 0 + state at LHC consistent in its properties with the SM Higgs boson, and the lack of discovery of other states proximate in mass to the SM states, implies that the linear SMEFT is a useful and efficient formalism to study and constrain possible deviations from the SM. Determining the global constraints on L 6 is important to inform efforts to search for physics beyond the SM, and will also be a critical consistency check in the event that a beyond the SM state is discovered. 2 A serious challenge to developing the constraint picture in the general SMEFT is the presence of many unknown parameters. Further, an approach that is inconsistent when considering bounds, for cut off scales in the 3 TeV range has generally been pursued, as we will show. A key point in the inconsistency is that neglected theoretical errors of the SMEFT can be already dominant in some precisely measured observables, when performing global fits [27]. Unfortunately, if Λ 3 TeV, then it is also unlikely that the impact of corrections to SM predictions, expressed in terms of higher dimensional operators, will be experimentally observable in the near future. 3 As such, to develop applicable and useful constraints it is important to not neglect the theoretical errors we discuss.
In this paper we determine constraints on some parameters present in L 6 , being careful to ascribe a theoretical error for the various observables. Our approach to Electroweak data is strongly influenced by the pioneering results in refs. [28,29]. We incorporate results on scattering data from the detectors that operated at the LEPI, PEP, PETRA, SpS, Tevatron, TRISTAN and LEPII accelerator complexes, as well as low energy data from Atomic Parity Violation and Deep Inelastic Scattering measurements from CHARM, CDHS, CCFR, NuTeV, SLAC E158, eDIS and SAMPLE into a global linear SMEFT analysis.

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The outline of this paper is as follows. In section 2 we lay out our fit methodology, while defining our approach to theory errors. We then present directly in section 3 our main results concerning LEP data and our global analysis. Most of the details of the analysis are relegated to the appendix. Our notational conventions are defined in the appendix and in the companion paper ref. [27].
A summary of our main conclusions is as follows. The per-mille/few percent constraint hierarchy concerning experimental precision at LEPI and LEPII/LHC does not consistently translate into a hierarchy of constraints on individual leading Wilson coefficients in the SMEFT. Claims on per-mille, or sub-per-mille constraints on all individual L 6 parameters that contribute to LEPI data, are not supported by our results. As a consequence, it is in our view not justified to set these parameters to zero in LHC analyses. This is the case even before SMEFT theoretical errors are included. When these errors are added, the experimental hierarchy in precision is further undermined in its projection into the theoretical parameters. We find that it is important to include SMEFT theory errors when experimental precision reaches the percent level, and critical to include these errors for experimental bounds that report per-mille constraints, when interpreting these bounds model independently in the SMEFT. The differences in fit methodology, observables used, manner of making SM theoretical predictions, and our (more) consistent treatment of theoretical errors explains why our conclusions differ from past results.

Operator basis and power counting
We use the well defined operator basis given in ref. [4] when calculating. We canonically normalize the theory in unitary gauge, taking the theory to the mass eigenstates as in ref. [30]. For power counting, we use the most general naive power counting, simply suppressing all operators by the appropriate power of the cut off scale Λ. Although alternative schemes of power counting can be self consistent, they are also limited in their applicability.
We adopt the assumption of exact U(3) 5 symmetry in the SMEFT corrections. We also adopt the assumption that the Wilson coefficients in L 6 , and the loop improved electroweak couplingα, are real in the analyses we present. These assumptions should also be relaxed, if possible to do so in a consistent manner. For a recent effort aimed at relaxing the U(3) 5 assumption, see ref. [31].

Fit methodology
Consider a set of observables Ω O = {O i } i∈ 1,n . We denote the measured value of an observable asÔ i while its predicted value i.e its value in the SMEFT 4 is defined bȳ

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where C 6 is a Wilson coefficient of an operator in L 6 , while C 8 is a Wilson coefficient of an operator in L 8 etc. Note that the C 6 contain an implicit factor 1/Λ 2 . We will sometimes pull this factor out and will write it explicitly as C 6v2 T /Λ 2 . O i is the prediction of the observable in the SM. Here Ω C = {C k } with k ∈ 1, q is the set of Wilson coefficients contributing to the shifts of all the O i . Note that α i,k can be 0 since in general just a subset of the C k contribute to the shift of an observable O i . This notation is consistent with the conventions in ref. [27].
The measured valuesÔ i can be regarded as a gaussian variable centred about the predicted valueŌ i following the central limit theorem. Introducing the n dimensional vectorsÔ = (Ô 1 , . . . ,Ô n ) andŌ = (Ō 1 , . . . ,Ō n ) we can write the likelihood function which is just the joint probability distribution function (p.d.f), of these n gaussian distributions where V is the covariance matrix with elements with the ρ exp,th being the correlation matricies for the experimental and theoretical errors respectively. 5 We have denoted |V | the determinant of the covariance matrix. We separate the experimental and theory errors to avoid introducing incorrect correlation effects. The ∆ th i is defined as where ∆ exp i , ∆ i,SM , ∆ i,SM EF T corresponds respectively to the experimental, SM theoretical, and SMEFT theory error for the observableŌ i . Assuming the maximum is found at L(C i ) = L max the random variable λ defined as has a chi square distribution with number of degrees of freedom ν = r, where r is the number of actual fitted parameters. The value of r may differ from the total number of Wilson coefficients, which is dim(Ω C ) = q. In (2.5), χ 2 is expanded as using (2.1). 5 Formally the covariance matrix V depends on the neglected parameters in the expansion, including dependence on C 6 that is higher order in the power counting. In other words, the dependence on the parameters in the observables fit to is always highly non-linear. Our approach is to approximate all of this implicit dependence on the parameters in higher order terms in the EFT expansion with a numerical error assigned to V . We note that alternative procedures where the implicit dependence on the C6 parameters in ∆i is made explicit, are (possibly) also consistent.

Experimental errors and SM theory errors
In the following sections we specify our approach to the errors in the global analysis in detail. Our purpose is to make the analysis reproducible and transparent. When we estimate a SM theoretical error directly in this work, we distinguish these estimates with a superscript in the data tables.

LEP based data
Generally, the theoretical error for fitting in the SM is well known. For LEPI based data, SM theoretical errors were taken to be the ones defined in ref. [32] for Γ Z , σ had and R f and in ref. [33] for A FB . We have used the values of the input parameters specified in ref. [27] to generate predictions in the SM for the LEPII based measurements in tables 3, 5, 6, 8 using ZFITTER. Following ref. [34] we have assigned an error of 0.53% for σ(e + e − → µ + µ − ), 0.61% for σ(e + e − → τ + τ − ) and 0.23% for coloured final state pair production when producing the theoretical prediction with ZFITTER for LEPII data. We have assigned an error of 0.01 √ 2 multiplying the error of the cross section σ e + e − →µ + µ − (resp. σ e + e − →τ + τ − ) for A µ FB (resp. A τ FB ) dropping the percentage symbol. This error prescription follows the discussion in ref. [34]. When the flavour universal BSM case is considered, the weighted least squares average of the σ(e + e − → µ + µ − ) and σ(e + e − → τ + τ − ) and of A µ FB and A τ FB were taken. We have also checked that the error introduced by propagating the SM errors in the input observables is subdominant to the estimated theoretical error in the SM already included, and specified below for LEPII observables. 6 In the calculation of 2 → 2 scatterings the fermion masses are frequently neglected. The largest error of this form effecting the fit comes about when considering the pair production of b quarks, and interference with the higher dimensional operators. However in this case this theoretical error is subdominant to the errors that are included in our theory error in the SMEFT defined below.

TRISTAN, PEP and PETRA
Measurements at energies below the Z pole are of interest when developing the global constraint picture. Different operating energies ( √ s), help resolve the large number of effects that are present when considering e + e − → ff scattering observables.
A challenge to using this data is the legacy theory predictions that the measurements are compared to. For example, consider the results for the TOPAZ collaboration. In ref. [35] R qq = σ(e + e − → qq)/σ(e + e − → had) and A F B q for q = b, c are reported at the operating energy √ s = 58 GeV with a full (experimental) correlation matrix. The SM predictions compared to are leading order predictions, with no theoretical error stated. Reproducing the predictions for R qq and A F B q with current PDG values of input parameters introduces shifts compared to the quoted theoretical value ∼ 1 σ for the experimental error quoted for R qq . However, the SM predictions are also corrected in a detector and decay mode specific manner [35]. As such, although leading order QCD radiative corrections are modelled with Monte-Carlo tools using JETSET7.3, we consider it reasonable to ascribe a ∼ 1% SM theoretical error, and to use the supplied predictions.

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The justification of a ∼ 1 % error assignment is that α s ( √ s 58 GeV)/4π ∼ 1%. We assume residual SM theory errors on the modelling of the leading QCD perturbative corrections for quark final state observables at TRISTAN, PEP and PETRA based detectors of this form. For leptonic final states we take a theoretical error estimate of ∼ 1% for cross section measurements and ∼ 0.1% for A F B measurements, in line with the theory errors produced for similar LEPII observables using ZFITTER. In all cases where we estimate a theory error for √ s <m Z colliders the error is subdominant to the experimental errors. In the case of TRISTAN, PEP and PETRA the theory error due to the SMEFT generalization of the SM is also expected to be far smaller than the experimental errors. This is however not the case for LEPI measurements.

Correlations
The theoretical correlations are essentially unknown. The experimental correlations between observables are frequently unknown, except in some exceptional circumstances. This limits how precisely leading parameters can be bounded in the SMEFT, although this effect is difficult to quantify. The well measured subset of LEPI data that define the well known LEPI pseudo-observables supply some correlations, which we use. We also use correlations for σ had supplied for LEPII data, and correlations supplied in ref. [35] for TOPAZ data. We also use correlations for reported low energy couplings g 2 L/R given in ref. [36].

LEP, TRISTAN, PEP and PETRA
It is also important to include a theoretical error estimate, due to the SMEFT itself [27]. This is in addition to the SM theoretical error. In the SMEFT, when obtaining a bound on an unknown Wilson coefficient in L 6 , the following effects are generally neglected: • Initial and final state radiation effects in the correction to 2 → 2 scattering. These corrections still have an approximate universal form [34,37,38] for observables O i . Here E γ max is the maximum photon energy not removed with isolation cuts on the signal, and E beam = √ s is the operating energy. Using the numerical results in ref. [34] (table 12) as a guide we estimate Λ 2 for lepton pair production, (2.8) Λ 2 for quark pair production.
• Neglected perturbative corrections in the SMEFT. These corrections are currently treated inconsistently in global fits. This requires the introduction of a theoretical error, which we define as

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Although the value of b for specific observables can be (mostly) inferred from the Renormalization Group (RG) results for the SMEFT in ref. [30,39,40], the corresponding "a" finite terms are not small enough in general to be neglected at NLO, see refs. [41][42][43]. Here µ 1,2 are schematic for the characteristic scales. Taking µ 1 = Λ, µ 2 = v, a = b = 1 and g = 0.65 for EW corrections we find an estimate for neglected running effects in the SMEFT As well as running down from a high scale, there is also the neglect of perturbative corrections in relating input observables to predictions around the electroweak scale. This can correspond to, for example, a scale characterising a low energy measurement of G F in µ − → e − +ν e + ν µ decay (∼ 10 GeV) compared to a characteristic scale √ s ∼ 190 GeV in a prediction using this measurement. Taking µ 2 = 10 GeV, µ 1 = v, a = b = 1 and g = 0.65 we get (2.11) • Corrections due to L 8 . These corrections introduce a theoretical error Although it is possible to consider some corrections due to L 8 to be absorbed into the definition of the effective parameter constrained in a measurement, using this constraint in an alternative process with different corrections due to L 8 makes this redefinition inadvisable.
Some O(v 4 /Λ 4 ) terms in the χ 2 are of particular concern. Consider expanding the prediction for an observableŌ i to second order In expanding a χ 2 function, ζ i,k,l terms, which exist in general at tree level, 7 are the same order as the terms in a χ 2 function that dictate the global minimum for the L 6 parameters C i , and hence the confidence regions. These ζ terms are of power counting order L 8 but they are potentially more problematic than new dimension eight operators for consistent fit efforts. The reason is that these terms contribute to the Hessian matrix that defines the global minimum. As the ζ terms are unknown, this matrix is formally undetermined at O(v 4 T /Λ 4 ) in the χ 2 , for fitting the parameters in L 6 .
Here F is an unknown scaling factor for the effect of these corrections in the off the Z pole LEPI data included in global analyses. This correction factor is difficult to quantify, but can be taken to be ∼ 40 pb −1 /155 pb −1 as a rough approximation. For cross section measurements this error can be neglected, see ref. [27] for a detailed discussion.
The number of operators in L 6 and L 8 leading to ∆ P , ∆ P,II , ∆ offshell,O i , ∆ L 8 is large. 8 It is reasonable to consider these corrections added in quadrature when considering the SMEFT theory error metric so that ∆ P , ∆ P,II multiply a further numerical factor √ N 6 , which is an order one number characterizing the number of L 6 operators that contribute. We also multiply the error due to the neglect of L 8 by an order one number √ N 8 for this reason. We absorb these factors into the definition of the theoretical error.
Adding these sources of theoretical error in quadrature defines a theory error metric When considering detectors operating off the Z pole, the contribution from ∆ offshell,O i can be neglected. Generally, at low Λ the neglect of L 8 dominates, while as Λ gets larger, the neglect of RG perturbative corrections begins to dominate. A reasonable approximation is given by The left plot shows the generic impact on percent and per-mille bounds experimentally, while the right shows specific LEPI observables compared to theory error. The actual impact of neglected terms depends strongly on the particular UV scenario integrated out. It seems reasonable to neglect ∆ i SMEFT when considering LEPI data only when very large cut off scales are implicitly assumed. The SMEFT is not currently developed to a level that allows a consistent incorporation of LEPI data if the SMEFT theory error is not included, for cut off scales Λ 3 TeV.
LEPI include the Z width (Γ Z ) which has a precision Whether ∆ i SMEFT is negligible, or dominant when considering an observable, depends upon the implicit assumptions about Λ adopted in a SMEFT fit, see figure 1. ∆ i SMEFT corresponds to a theoretical error "wall" on how precisely some SMEFT corrections can be currently bounded. This is particularly the case for the most precise LEPI observables, which are per-mille constraints -experimentally.
It is possible in some UV scenarios that our power counting assumption essentially does not apply. We have made the simplifying choice to suppress all operators by the same scale Λ, for illustrative results, to determine in some simple cases how large an impact SMEFT theory errors have.

Low energy measurements
For measurements at effective scales µ 2 v 2 T it is appropriate to integrate out the Higgs, top, W, Z bosons etc. and transition to a general low(er) energy SM EFT (denoted SMeFT). Below the mass scales of these states the operators present in the Effective Lagrangians we will consider run according to the Renormalization group equations in the SMeFT,

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determined with no propagating states with masses ∼v T . 9 We are neglecting these running effects (as well as the threshold matching corrections) which necessitates introducing another theoretical error. These corrections lead to theoretical errors on the order of on the coefficient of the low energy operator in the Effective Lagrangian, when a low scale measurement is made at s ∼ Q 2 . Higher order terms in the expansion of Q 2 /m 2 Z are neglected, with give a much smaller error O(10 −6 ), for Q 1 GeV. Although the running of the lower energy operators can be incorporated directly, the resulting reduction in the theoretical error is not substantial, until L 8 is known. This is because at the threshold when matching the linear SMEFT to the SMeFT at s ∼v 2 T , unknown terms in SMEFT of the form (ψD µ ψ)(ψD µ ψ) (for example) are present. These operators can give tree level matching corrections that are on the order of O(v 2 T /Λ 2 ) to the effective operators considered in the lower energy theory. For Λ ∼ TeV, the resulting theoretical errors on the effective Wilson coefficients are comparable to ∆ SMeFT . The situation changes once L 8 is known, and more precise bounds can be pursued. The SMEFT error metric for low energy measurements is approximated as

Impact of reducing ∆ SMEFT
The impact of systematically improving the SMEFT predictions, and the sensitivity of bounds on coefficients in L 6 to theory errors is a subject of some debate in the literature currently, following the stressing of these issues in ref. [27]. It is subtle to correctly characterize the impact of neglected effects and theoretical errors for the following reason. Consider the effect of changing an error in the fit when ∆ SMEFT becomes dominant, as in the case of some LEPI observables with a lower cut off scale. For example, consider changing the theory error on the W mass from ∆ M W ∼ 0.2% (including ∆ SMEFT ) to ∆ M W ∼ 0.02% (neglecting ∆ SMEFT ). The later value is the quoted theory error in the SM alone. The χ 2 function constructed will then be modified with some terms obtaining corrections of the form Such changes to the most precisely measured observables do not have a negligible effect on the confidence regions obtained, see section 3. It is reasonable to attempt to characterize the effect of neglected higher order terms and corrections by expanding the likelihood in the correction to the observables. Then one obtains a modification of the form For an example of an analysis of this form see ref. [44].

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to the χ 2 when neglecting correlations between the different observables. These effects are numerically suppressed relative to χ 2 terms of the form The numerical suppression is due to the fact that Ô − O i ∼ ∆ i so that a relative suppression by ∆ i is numerically present when considering ζ i,k,l , γ i,k ∼ 1. 10 This can lead to numerical behavior that indicates that these terms have a small effect on the likelihood. Studying this issue without simultaneously changing the theory error in the fit (i.e while neglecting the effects of the changes in eq. (2.23)) leads to the wrong conclusion on the sensitivity of the fit to higher order effects. This error has been very frequently made in the literature.
It is important to stress that ∆ SMEFT can be systematically reduced, if more sophisticated theoretical predictions are developed. It is essential that a non redundant and well defined basis of L 8 be determined. 11 Perturbative corrections to one loop order for L 6 operators are also required to be systematically determined and included in the SMEFT, to advance the effort to reduce the (potentially) dominant theoretical errors. 12

Numerical results
The appendix contains details on the data and theoretical calculations used to perform the global fit. In this section we present our results.

LEPI results
We use the systematic results in ref. [27] for redefining the input observables in the SMEFT and making LEPI predictions. The data and theory predictions in the SM are given in table 5. We present two results, one applicable for lower cut off scales (Λ 3 TeV), where the error in observables that are more than percent level precise is assumed to be dominated by ∆ SMEFT,i , and one applicable for larger cut off scales where ∆ SMEFT,i is neglected. In the second case, we find Hl , C Hl , C Hq , C Hq , C ll , C HW B , C HD },

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and M LEPI is given by The M LEPI matrix is symmetric so the lower triangular entries are not shown. For lower cut off scales (Λ 3 TeV) we introduce a common ∆ SMEFT,i ∼ ∆. We further approximate ∆ ∼ 0.3% following the discussion in section 2.4.1. In this case, this error will significantly affect the impact of the measurements R , σ had , Γ Z , M W on the fit space. To illustrate the impact of theory error. We find the LEPI constraint χ 2 function is Comparing χ 2,<3Tev LEPI and χ 2 LEPI we see that the impact of theory error is not negligible. To further visually illustrate the impact of accounting for theoretical errors in LEPI data we take the results for χ 2 LEPI and compare the constraints for a χ 2 function developed with a varying ∆ SMEFT = {0.3%, 1%}. Figure 2. The effect of varying ∆ SMEFT on an oblique analysis. The green, yellow, grey regions correspond to the 68%, 95% and 99.9% CL regions for a two parameter fit around the minimum of the χ 2 distribution. The regions correspond to χ 2 = χ 2 min + ∆χ 2 with ∆χ 2 = 2.30 (1σ, green), 6.18 (2σ,yellow), 11.83 (3σ, grey) defined via the Cummulative Distribution function for a two parameter fit. The left plot does not include any theory error for the EFT, the middle sets ∆ SMEFT ∼ 0.3%, the right sets ∆ SMEFT ∼ 1%.

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To make the comparison easy to interpret we show the dependence on a subset of Wilson coefficients. We plot the confidence regions about the χ 2 minimum setting all parameters other than those corresponding to the S, T parameters to zero. We use the normalization This case corresponds to a traditional oblique S, T fit in EWPD, following the formalism of refs. [46][47][48][49]. The impact of ∆ SMEFT is shown in figure 2. The plots shown can be understood as relaxing the defining assumption of an oblique analysis, that all SMEFT parameters other than S, T vanish. This defining assumption is not RGE invariant (and challenged by field redefinitions in the SMEFT [21,50]), so it is clearly relaxed in a more consistent analysis. We also show in the following section the effect of profiling away all other parameters other than S, T , which further increases the confidence level regions. However, the results obtained in the two cases should only be compared with caution, as they correspond to two different defining conditions for the confidence level regions. In figure 3 the impact of varying ∆ SMEFT on the bounds of the Z ff vertex operators C He , C Hq is shown. We also show the confidence levels for the two parameters C He and C We do not find that all individual Z ¯ couplings due to L 6 (such as C Hev 2 T /Λ 2 ) are constrained at the per-mille, or sub-per-mille level in a completely model independent fashion. If bounds on deviations are to be completely model independent when the SMEFT is assumed, then the case where ∆ i SMEFT is dictated by a low cut off scale (Λ ∼ 1 − 3 TeV) JHEP02(2016)069 must be accommodated. As a result, the case where ∆ SMEFT is not negligible is always relevant for a model independent constraint. The case where the cut off scale is not too large, and patterns of deviations can be measurable, is also the case where global fits are of most interest.
The plot results shown assume that the "correct" global minimum is obtained in the χ 2 distribution when determining the confidence regions of the parameters in L 6 . There is ample reason to expect this to not be the case, see ref. [27] for some discussion on this point. Again we stress that the Hessian matrix that defines the global minima is formally undetermined at O(v 4 T /Λ 4 ) in the χ 2 for fits to parameters in L 6 . It is important to calculate the ζ terms in the SMEFT for precisely measured observables for this reason.

Global fit results
The global fit of all observables listed in the appendix has nineteen Wilson coefficients and a total of one hundred and three observables. When considering the global analysis, r = 17 when our fitting assumptions 14 are adopted. Our approach to the remaining flat directions is to fix the sum of the null vectors of the fit space to their power counting size in a manner consistent with the error assigned. This introduces two auxiliary conditions on the fit that are fixed tov 2 A simultaneous global analysis involving the observables considered here, and measurements of exclusive W pair production processes (while no parameters in the SMEFT are set to zero) is expected to fix these flat directions to a size consistent with the theoretical error determined by the power counting. In the absence of such a truly global analysis, we fix the flat directions to not be zero, but to a value consistent with their power counting size and the ∆ SMEFT assumed, as a reasonable approximation.

Profiling to lower dimensional fit spaces
The constraints on each C i G when C j =i G is profiled over is of some interest in building intuition on the model independent degree of constraint. However, we caution that considering constraints on individual parameters while profiling, as opposed to the constrained Eigenvectors (of the Fisher matrix) can also be misleading.
We calculate the χ 2 and express it as where C G,min corresponds to the Wilson coefficients vector minimizing the χ 2 G and I is the Fisher information matrix.
To profile away parameters C i/ ∈ 1,n G,min and retain dependence on C i G with i ∈ 1, n , we introduce the vectors We denote by C ⊥,min,P the vector C ⊥ that minimizes the χ 2 when the n parameters C i are free. Note that C ⊥,min = C ⊥,min,P but are related by the following formula where I ⊥ ,Ĩ and I all correspond to the components of I defined as Calculating C ⊥,min,P using (3.9) and using its value in χ 2 G (C G ), we get the profiled χ 2 P C that only depends on the remaining n parameters C i . To get a constraint on one Wilson coefficient C I G , we profile away all other Wilson coefficients as described above taking the particular case n = 1. Then, using χ 2 P C = C I G , we calculate the 1σ confidence level region for C I G as usual. We repeated this procedure for a SMEFT error equals to {0%, 0.1%, 0.3%, 0.5%, 1%} and for each value taken, we quote χ 2 G,min , C G,min ± σ as well as the full Fisher information matrix I in the appendix. We give the C G,min ± σ in table 1, which shows O(%) or O(10%) constraints on the individual C i G . Taking n = 2 we obtain a two parameter fit for Wilson coefficients we are interested in. We plot an nontraditional S, T result -where all others parameters than S, T are profiled away and not taken to zero -for different values of the SMEFT error: {0%, 0.3%, 1%} in figure 4. These confidence regions should be interpreted with care. In a well defined model in the UV, a set of predictions for all the C i G will be present. Such a model leads to relations between the Wilson coefficients, that need to be imposed on the global fit space. Note that the global JHEP02(2016)069  results given in the appendix, has been minimized with respect to the C i G , treating the C i G as free parameters. The parameters profiled away can still lead to a model being excluded, even if the remaining parameters in the low energy limit of the model are consistent with the confidence regions shown in figure 4, 5. This is due to the fact that these confidence regions are valid when the parameters profiled away are treated as free. Further, we note that the S, T result in figure 4 should only be compared with caution to figure 2, due to the different assumptions employed in the analyses. Nevertheless, it is still interesting that relaxing the strict assumptions of an oblique analysis (that all parameters other than S, T are neglected) will generally lead to a degree of constraint that is in between the constraints shown in figure 2 and figure 4. We also follow this procedure for the two parameters C He and C Hq to compare with figure 3 and find the result in figure 5. However, we note again that this comparison requires significant caution in interpretation.  Table 1. Shown are the best fit points of the C i G and the one sigma error as a function of ∆ SMEFT . Here we have profiled over all C j =i G to reduce to a one dimensional fit space. The columns are labeled as (1σ, ∆ SMEFT ). The Wilson coefficients have been scaled asC i G = 100 C i G where C i G contains an implicit factorv 2 T /Λ 2 . As expected the consistent introduction of a theoretical error does relax the bounds on the C i G . Note that even when ∆ SMEFT = 0, individual operators that contribute to δ(Z¯ ) are only model independently constrained at the percent level. Constraints on some four fermion operators are an order of magnitude weaker for the data considered.

The eigensystem of the global fit
The degree of constraint on orthogonal linear independent combinations of the Wilson coefficients (denoted W ∆ SMEFT k ) significantly varies for the global fit. Here k = 1 . . . 19 sums over all of the orthogonal eigenvectors (of the Fisher matrix I) in our global fit. The normalized Eigenvectors and Eigenvalues of the system are directly obtained from the Fisher matricies given in the appendix. The Eigenvectors are normalized so that The bands are ∆ SMEFT = 1%, 0.3%, 0% for the brown, green and blue lines respectively. We show results left to right for fixing the auxiliary constraint lifting the two flat directions to bev 2 T /2Λ 2 ,v 2 T /Λ 2 and 2v 2 T /Λ 2 , treated as an error.  As  Figure 8. Here, the focus is on the Wilson coefficients contributing to the Z ¯ coupling redefinition. We show how the SMEFT error affects the constraints on these Wilson coefficients.
The green band corresponds to having C i G constrained to a per mill level < 1%. We show results left to right for fixing the auxiliary constraint lifting the two flat directions tov 2 T /2Λ 2 ,v 2 T /Λ 2 and 2v 2 T /Λ 2 , treated as an error.
scale. The results show that the hierarchy of constraints is roughly dictated by LEPI observables, as expected, and these constraints are also relaxed when theory error is consistently included. Small changes in theory errors can have a dramatic impact on the most constrained Eigenvectors; for example, they change the scale of suppression on the most constrained Eigenvector by 8 TeV. There are six individual Wilson coefficients that effectively lead to anomalous couplings of the form δ(Z µ¯ γ µ ): C HW B , C HD , C l l , C He , C Hl , C Hl . The six most constrained Eigenvectors do not only involve these parameters in a numerically dominant fashion, as we have explicitly verified. This can be directly checked by using the Fisher matricies supplied in the appendix. This is the case if ∆ SMEFT is neglected, or not.
The most strongly constrained Eigenvector is (approximately) Hl + 4.7 C (1) This (approximate) Eigenvector remains constrained as ∆ SMEFT is not neglected, for example Hl + 4.8 C It is easy to understand the appearance of C Hq , which gives contribution to the Z coupling to quarks, in the most constrained Eigenvector. LEPI data on the partial widths are inferred from the measurements of the pseudo-observable ratio R 0 f , that always involve the couplings of the Z to quarks.
It is reasonable to impose the global fit constraints for pre-LHC data on LHC studies, when considering possible deviations allowed in the SMEFT. 15  effective scale in an experiment is µ ∼m Z the Eigenvector W 1 is highly constrained. 16 This is not equivalent to just setting δ(Z µ¯ γ µ ) = 0.
To optimally incorporate the constrains from global fits that include more pre-LHC data, or LHC data from Run1, this point still holds. The Eigenvectors and Eigenvalues of the system are sensitive to the full set of measurements that are required to fully constrain the Wilson coefficient space model independently.

Conclusions
We have developed the global constraints of the SMEFT considering data from many (pre-LHC) experiments. We have also developed a theory error metric, and used this result in the global fit. We believe our results demonstrate that SMEFT theory errors should not be neglected in future fit efforts.
Our conclusions differ somewhat from recent claims in the literature. We find that the per-mille/few percent constraint hierarchy concerning experimental precision at LEPI and LEPII/LHC does not consistently translate into a hierarchy of constraints on individual 16 The requirement that the scale be µ ∼mZ is due to the fact that the Eigenvector is not preserved under RG evolution.

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leading Wilson coefficients in the SMEFT. Due to this, we stress again that, it is in our view not justified to set individual Wilson coefficients to zero in LHC analyses to attempt to incorporate pre-LHC data in the SMEFT. This is the case even before SMEFT theoretical errors are included. When these errors are added, this point is only strengthened.
Relaxing bounds on a number of unknown parameters in a global fit from the per-mille level to the few percent level is more significant than naively expected. This is because exactly this hierarchy of constraints has been used to neglect parameters in other LHC studies using the SMEFT. Inconsistent approaches to the linear SMEFT could in time lead to an incorrect conclusion that the linear SMEFT has to be abandoned, in favour of the more general nonlinear formulation. As such, obtaining precise, consistent, and reproducible bounds on the SMEFT is essential.
The differences in fit methodology, observables used, SM theoretical predictions, and our treatment of theoretical errors explains why our conclusions differ from past results. We have supplied significant details on our results to make our conclusions reproducible. These details are presented in the appendix. We will supply the main result of the global fit likelihood (as a function of the cut off scale) in a mathematica file, upon request, to aid in reproducing our results.

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also include the definition of the operator basis we use [4] in this appendix for completeness.
Hq pr and δ(g   Table 2. Experimental and theoretical values of the σ e + e − →ff in pb. Note that R exp/th is the quoted ratio of the experimental cross section with the SM theoretical prediction from ref. [57,58]. Theoretical errors are included in the quoted error for this ratio. When we construct theoretical predictions using ZFITTER, we follow the guidance of ref. [52] and use the input observable values quoted in ref. [27]. We discuss our approach to theoretical errors, including errors for the SMEFT theoretical framework itself, in section 2. With the simplifying assumptions of total U(5) 5 symmetry in the effects of L 6 , real wilson coefficients and a narrow width approximation for the shifts (neglecting terms or order Γ Z /v in the shifts, but not the error ∆ SMEFT,i ), we find the result for differential + − → ff scattering

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while some contributions to the forward-backward asymmetries are proportional to For the detectors taking data at the TRISTAN accelerator (AMY,VENUS and TOPAZ) we approximate the angular acceptance by −0.6 ≤ cos θ ≤ 0.6 17 giving the weighted contributions For PEP and PETRA, a reasonable approximation for the angular acceptance is | cos θ| < 0.80 which is an average of the one used for muon and tau final state pair production. The angular acceptance of the LEP experiments is superior but varies between the experiments. As a reasonable approximation we use the angular acceptance of −0.9 ≤ cos θ ≤ 0.9. This choice is informed by ref. [52].

B.1.1 Forward-backward asymmetries for u, d,
The shift in the FB Asymmetries off the Z pole are obtained from the general formula Where we can calculate δ(σ e + e − →ff ) F −B and use our previous expression for δσ e + e − →ff to get the full expression of δA 0,f FB . For FB asymmetries near the Z pole, the previous expression simplifies to   The shift in the e + e − → e + e − differential cross section differs from the case of e + e − →f f . In the limit of a vectorial coupling, and neglecting the mass of the vector boson, the structure of the equations describing Bhabba scattering [69] is well known. In this limit, a s ↔ t interchange symmetry that corresponds to the indistinguishability of the initial and final state particles is present. We structure our presentation of the shift in Bhabba scattering to reflect this limit finding

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Where we have introduced We use the LEPII data given in table 9 for Bhabba scattering, which is a subset of LEP data. We have examined the bin dependence of the shifts in the SMEFT and chosen the bins in table 9 to optimise sensitivity to possible shifts, while not oversampling Bhabba scattering data. This choice is driven by the fact that the Bhabba scattering data does not supply a correlation matrix.

C Low energy precision measurements
Due to the large number of operators contributing in a general analysis of LEP data, and related 2 → 2 scattering data at lower energy colliders, it is of interest to extract constraints from yet other measurements. A useful source of information is to also incorporate bounds from neutrino Deep Inelastic Scattering (DIS) experiments. We utilize bounds from neutrino-electron (CHARM and CHARM II [72,73], and CALO [74]) and neutrino-nucleon scattering (at CDHS [75], CHARM [72], CCFR [76], and NuTeV [36]) experiments. From inelastic electron scattering (at SLAC E158 [77]) we incorporate bounds from low energy parity violating asymmetry measurements. Using data from polarized electron scattering experiments at SLAC (eDIS [78]) and the SAMPLE experiment [79] we extract bounds from Atomic Parity Violation measurements.

C.1 ν lepton scattering
For ν e ± → ν e ± scattering we calculate the shift ofḡ νe V,A , where these parameters are defined by the following Effective Lagrangian SM Value Ref. Table 9. Experimental and theoretical values of the LEPII observables σ e + e − →e + e − . For a theory error we take 0.2% for the legacy LEPII data, following the discussion in ref. [71].
Recalling that δg ν V = δg ν A , g x V = T 3 2 − Q x s 2 θ , g x A = T 3 2 and g ,W V,A = 1 2 , the shifts are then these shifts add the contributions of W and Z exchange. Depending on the neutrino flavour some terms are absent. The shift that is relevant for g νµe A,V does not have a δM 2 W or δg ,W ± V,A contribution, whereas a shift for g νµµ A,V has both contributions. We use the later for neutrino trident production. We use the former for fitting to the data in table 10 to constrain these shifts.

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Obs.  Table 10. Experimental and theoretical values of g νe V and g νe A . The theoretical prediction and error is taken from ref. [81] and is estimated by the leading Q dependent neglected correction, which is quoted as two orders of magnitude below ±0.02.

C.2 ν nucleon scattering
For ν N → ν X scattering, we consider a Z exchange in the SMEFT. We define two parameters¯ q L and¯ q R for q=u,d by the following Effective Lagrangian are the Z couplings of the quark. The redefinition of the Z couplings and the corrections due to ψ 4 operators lead to a shift in q L and q R of the form¯ q L/R = q L/R + δ q L/R with δ q L/R given for up and down quarks Here we used δg ν V = δg ν A and G ν V = G ν A = 1 4 . In terms of some common notation used in ref. [33,81] For ν N → X and the inverse process, W exchange definesΣ ij L by the following Lagrangian where for the tree level SM result (Σ ij L ) SM = V ij CKM , where V CKM is the Cabibbo-Kobyashi-Maskawa matrix. (Σ ij L ) SM receives corrections from W couplings redefinitions and the M W redefinition, so thatΣ ij L = (Σ ij L ) SM + δΣ ij L with

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Where we used that δg x,W V = δg x,W A . In principle one can include in the Lagrangian a term of the formΣ ij R , with a right handed projector. This term is zero in the SM, but can be generated by the operator Q edq in the SMEFT. These corrections are proportional to Yukawa terms and so vanish when we consider massless fermions, and are neglected.
Analyses of ν Nucleon scattering rely on relations between charged and neutral current process parameterizing effective left and right handed couplings on Isoscalar targets [82] for the scattering variables defined in terms of the momentum transfer q 2 , the nucleon momentum p N and the neutrino momentum p ν . These effective couplings receive corrections in the SMEFT so that g 2 L/R,eff = g 2 L/R,eff + δg 2 L/R,eff and (C.14) Although these expressions are general for all flavours, we will implicitly restrict our attention to the case of only first generation quarks in the target nucleon when considering PDFs. Data on ν Nucleon scattering tends to be reported as a ratio of cross sections The factor r in an ideal experiment with full acceptance (in the absence of sea quarks) is given by r = 1/3. When fitting shifts to the SM expectation we use a supplied value of r if it is simultaneously fit to, as in the case of CHARM [72]. Otherwise we use r ∼ 0.44. In principle further corrections in the SMEFT can be present in r. Here we have assumed that the effect of the SMEFT on the parton and anti-parton distributions of the neutrons and protons is negligible compared to the corrections that we include in eq. (C.4), (C.10). This choice is motivated out of our adoption of a U(3) 5 scenario, and the neglect of the flavour violating effects of L 4 feeding into L 6 . These assumptions, and the implicit assumption that these corrections scale as Λ 2 QCD /Λ 2 , motivate neglecting these effects. This introduces a further theoretical error of the form This error is neglected in the fit. CCFR reports data in terms of the parameter κ which is given by We use the data given in  Table 11. Experimental and theoretical values of R ν and Rν. Theory predictions are obtained by using the leading order Llewellyn-Smith relations with a fitted r in the case of CHARM, with input parameters for the SM g L,R as quoted in the PDG [33]. Similarly the relation reported in eq. (C.17) is used with input values for g L,R , h L,R taken from the PDG for κ. The NuTeV results are also compared to the quoted g L,R values from the PDG. The theoretical predictions for ν Nucleon scattering are subject to theoretical uncertainties due to higher order neglected corrections in perturbation theory (beyond one loop order generally) and harder to quantify PDF and nuclear form factor uncertainties. As the determined value of r feeds into the theoretical prediction for CHARM which has errors of a few percent we take this as the dominant theoretical error. The CCFR collaboration quoted a SM prediction [76] with 0.2% theoretical error. We use this value in the modified theory prediction used. The interpretation of the NuTeV result is potentially subject to large uncertainties as detailed in the PDG [33]. We assign the neglected isospin violating PDF correction (detailed in ref. [83], eq. (34)) as a theory error.

C.2.1 Neutrino trident production
Neutrino trident production is the pair production of leptons from the scattering of a neutrino off the Coulomb field of a nucleus, ν N → ν N + − . The scattering of such highly relativistic neutrinos is well approximated by the Equivalent Photon Approximation (EPA) [84,85] and has been recently discussed in the context of Z models in refs. [86,87]. The SM calculation of this process is well known, see refs. [88,89]. Here we follow the discussion and notation in ref. [87,88]. The effective Lagrangian for this interaction is given by eq. (C.1). The constraint on the SMEFT is through the ratio of the partonic cross sections As the effects we consider are heavier than the SM W, Z bosons, we assume that the subsequent phase space integrals over the partonic process are not modified. Due to this assumption we can directly constrain this ratio with the entries in table 12. Note that at tree level in the SM (g νee V ) SM = 1 2 + 2 s 2 θ and (g νee A ) SM = 1 2 . We expand out to linear order in the shifts δg νee V , δg νee A when constraining this ratio.

C.3 Atomic Parity Violation
For Atomic Parity Violation (APV) the standard Effective Lagrangian is given by qḡ eq AV ēγ µ γ 5 e (qγ µ q) +ḡ eq V A (ēγ µ e) qγ µ γ 5 q , (C. 19) JHEP02 (2016) Table 12. Experimental and theoretical values of Neutrino trident production, as a ratio to the SM cross section. Due to the variation in the reported NuTeV results, depending on the background treatment, we do not include the NuTeV result in the fit. The effective energy transfer in Neutrino trident production is a fraction of the Neutrino beam energy quoted, so that using an effective lagrangian is justified. Theoretical errors have been absorbed into the error on the quoted ratio in this case, and we assume that the extra SMEFT error is subdominant to the ∼ 35% error in the reported ratios.
Where in the SM we have (g eq We are interested in the corrections that g eq AV and g eq V A get when q = u, d. The effective shifts are From these four couplings we define a set of four others couplingsḡ ep AV /V A = 2ḡ eu AV /V A + g ed AV /V A andḡ en AV =ḡ eu AV /V A + 2ḡ ed AV /V A . These new couplings are shifted from their SM values by We then define the weak charge Q Z,N W of an element X A Z by [33,81,92] Q Z,N W = −2 Z g ep AV + 0.00005 + N (g en We use the precise determinations of Q Z,N W for Thallium(TI) and Cesium (Cs) given in table 13 to construct constraints from these measurements.

C.4 Parity violating asymmetry in eDIS
For inelastic polarized electron scattering e L,R N → e X the right-left asymmetry A is defined as [33]: Moving to the SMEFT, g eq AV /V A get corrected so that:ḡ eq AV /V A = g eq AV /V A + δg eq AV /V A so that a 1 and a 2 receive the corrections We use the data in table 14 to bound deviations in eDIS experiments. These results are again subject to theoretical uncertaintes in the form of isospin violating effects, nuclear form factors, etc. For example, measurements of inelastic electron scattering are also sensitive to the magnetic strange quark form factor. The SAMPLE experiments [79,96] measured the parity-violating asymmetry A for different momentum transfer Q 2 and different targets. SAMPLE I were performed on a Hydrogen target, while SAMPLE II was performed on a deuterium target, both at Q 2 = 0.1. The first two SAMPLE measurements allow an extraction of the magnetic strange quark form factor which is then used in SAMPLE III, carried out on deuterium targets, but at Q 2 = 0.038(GeV/c) 2 . The results from the HAPPEx experiments [97] are not used as the SM is assumed in their analysis [81]. Similar comments apply to the results of the PVA4 measurements at the MAMI microton.

C.5 Møller scattering
For the Parity Violation Asymmetry (A P V ) in Møller scattering, we use the standard Effective Lagrangian  A P V 0.2GeV (−131 ± 14 ± 10) × 10 −9 [77] (−126 ± 2) × 10 −9 [77]  The constraints on A P V are determined by examining fixed target polarized Møller scattering data (e − e − → e − e − ). In the SM we have g ee In the SMEFT we have the correction The parity violating asymmetry A P V is then expressed as (C.36) Here Q 2 ≥ 0 is the momentum transfer and y is the fractional energy transfer in the scattering y Q 2 /s. The SLAC E158 experiment [77] measured Møller scattering at Q 2 = 0.026GeV 2 reporting A P V = (−131 ± 14 ± 10) × 10 −9 .

D Universality in β decays
As discussed in ref. [51] in a model independent context, 18 it is possible to place bounds on combinations of four fermion operators and W ± vertex corrections by comparing the extraction of G F from µ − → e − +ν e +ν µ decays to its determined value in other semileptonic β decays. This constraint is presented in terms of a bound on the unitarity of the CKM matrix, assuming U(3) 5 universality in the SMEFT. We use the bound determined in ref. [100] for this purpose, which quotes after a careful examination of the (SM) theoretical and experimental errors present in the determination of the CKM matrix elements phenomenologically. Formally, the fit 18 Note this point was first stressed in the context of SUSY in ref. [99].

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performed in ref. [100] should be redone with the inclusion of a SMEFT error for each observable following the discussion in section 2.4.1. This is beyond the scope of this work, and as an approximation we add a numerical ∆ SMEFT error in quadrature with the quoted error above that is consistent with the theory error assigned to other observables, when performing the joint fit. This means that we treat this constraint, which is the result of a global fit of many observables, as a single net observable for constraints in the SMEFT. In the Warsaw basis, this constraint is a bound on the following combination of operators Hl . (D. 3)

E Global fit results
Considering now all the observables listed, a total 103 observables, the global fit result using the method described in section 2.2 is given as follows. In the global fit r = 19 = dim{C G } once the auxiliary conditions are imposed. Since our observables are shifted linearly in the Wilson coefficients, the Cramer-Rao bound is exact, meaning that the covariance matrix of our Wilson coefficients V C G is exactly given by V C G = I −1 . We give the Fisher information matrix as I ∆ SMEFT . Note that we have not included exclusive measurements of W pair production in this version of the fit. This is due to the severe challenge of properly incorporating these measurements in the SMEFT. Some of these challenges are discussed in ref. [21]. When these measurements are included, it is expected that the flat directions will be lifted. The ordering of the rows and columns of the Fisher matrix corresponds to the Wilson coefficient order in C G . We give the C G,min for ∆ SMEFT = {0, 0.1%, 0.3%, 0.5%, 1%} in table 1.

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Open Access. This article is distributed under the terms of the Creative Commons Attribution License (CC-BY 4.0), which permits any use, distribution and reproduction in any medium, provided the original author(s) and source are credited.