CP violating effects in coherent elastic neutrino-nucleus scattering processes

The presence of new neutrino-quark interactions can enhance, deplete or distort the coherent elastic neutrino-nucleus scattering (CEvNS) event rate. The new interactions may involve CP violating phases that can potentially affect these features. Assuming light vector mediators, we study the effects of CP violation on the CEvNS process in the COHERENT sodium-iodine, liquid argon and germanium detectors. We identify a region in parameter space for which the event rate always involves a dip and another one for which this is never the case. We show that the presence of a dip in the event rate spectrum can be used to constraint CP violating effects, in such a way that the larger the detector volume the tighter the constraints. Furthermore, it allows the reconstruction of the effective coupling responsible for the signal with an uncertainty determined by recoil energy resolution. In the region where no dip is present, we find that CP violating parameters can mimic the Standard Model CEvNS prediction or spectra induced by real parameters. We point out that the interpretation of CEvNS data in terms of a light vector mediator should take into account possible CP violating effects. Finally, we stress that our results are qualitatively applicable for CEvNS induced by solar or reactor neutrinos. Thus, the CP violating effects discussed here and their consequences should be taken into account as well in the analysis of data from multi-ton dark matter detectors or experiments such as CONUS, $\nu$-cleus or CONNIE.


I. INTRODUCTION
Coherent elastic neutrino-nucleus scattering (CEνNS) is a process that occurs when the de Broglie wavelength λ of the scattering process is larger than the nuclear radius. In terms of the exchanged momentum q this means that when q h/r N 100 MeV the individual nucleonic amplitudes sum up coherently. As a consequence the total amplitude gets enhanced by the number of nucleons, resulting in a rather sizable cross section. Indeed, among all possible scattering processes at neutrino energies below 100 MeV, CEνNS has the largest cross section. Measuring CEνNS however is challenging due to the small nuclear recoil energies involved. The first measurement was done in 2017 by the COHERENT experiment, which observed the process at a 6.7 σ confidence level (CL), using neutrinos produced in the Oak Ridge National Laboratory Spallation Neutron Source [1].
Given the constraints on the neutrino energy probe, CEνNS can be induced by neutrinos produced in fixed target experiments such as in COHERENT, reactor neutrinos and solar and atmospheric neutrinos. Within the second category CONUS is an ongoing experiment [2] and there are as well other experimental proposals that aim at using reactor neutrinos to measure CEνNS using different technologies [3,4]. Relevant for the third category are direct detection multi-ton dark matter (DM) experiments such as XENONnT, LZ and DAR-WIN [5][6][7]. There is clearly a great deal of experimental interest on CEνNS, in particular for the role it will play in nearfuture DM direct detection experiments [8,9] and the different physics opportunities it offers in these facilities [10][11][12][13][14][15][16]. * daristizabal@ulg.ac.be † deromeri@ific.uv.es ‡ nicolas.rojasro@usm.cl From the phenomenological point of view, it is therefore crucial to understand the different uncertainties the process involves and the impact that new physics effects might have on the predicted spectra. The Standard Model (SM) CEνNS cross section proceeds through a neutral current process [17,18] 1 . Depending on the target nucleus, in particular for heavy nuclei, it can involve sizable uncertainties arising mainly from the root-meansquare radius of the neutron density distribution [20]. However, apart from this nuclear physics effect the SM provides rather definitive predictions for CEνNS on different nuclear targets. Precise measurements of the process offer a tool that can be used to explore the presence of new physics effects. In fact, since the COHERENT data release [1,21], various analyses involving new physics have been carried out. The scenarios considered include effective neutrino non-standard interactions [22][23][24], light vector and scalar mediators [23,25], neutrino electromagnetic properties [26,27], sterile neutrinos [26] and neutrino generalized interactions [28].
Analyses of new physics so far have considered CP conserving physics. This is mainly motivated by simplicity andarguably-because at first sight one might think that getting information on CP violating interactions in CEνNS experiments is hard, if possible at all. CP violating effects are typically studied through observables that depend on asymmetries that involve states and anti-states or polarized beams, which in a CEνNS experiment are challenging to construct. In this paper we show that information on CP violating interactions can be obtained in a different way through the features they induce on the event rate spectrum, and for that aim we consider light vector mediator scenarios (with masses m V 100 MeV).
Phenomenologically, among the possible new degrees of freedom that can affect CEνNS, light vectors are probably the most suitable. In contrast to heavy vectors, they are readily reconcilable with constraints from the charged lepton sector, while at the same time leading to rather sizable effects [29]. In contrast to light scalar mediators, they interfere with the SM contribution and can eventually lead to a full cancellation of the event rate at a specific nuclear recoil energy. This is a feature of particular relevance in the identification of CP violating effects, as we will show.
In our analysis we use the COHERENT germanium (Ge), sodium (Na) and liquid argon (LAr) detectors to show the dependence of CP violating effects on target materials and detector volumes. We fix the detector parameters according to future prospects [30] and in each case we extract information of CP violation by comparing CP conserving and CP violating event rate spectra (induced by real or complex parameters). We then establish the reach of each detector to constrain CP violating effects by performing a χ 2 analysis.
The rest of the paper is organized as follows. In sec. II we fix the interactions, the notation and we introduce the parametrization that will be used throughout our analysis. In sec. III we present the parameter space analysis, we discuss constraints on light vector mediators and identify CP violating effects. In sec. IV we discuss the possible limits that the sodium, germanium and argon detectors could eventually establish on CP violating effects. Finally, in sec. V we summarize our results.

II. CP VIOLATING INTERACTIONS
Our analysis is done assuming that the new physics corresponds to the introduction of light vector mediators. This choice has to do with phenomenological constraints. Although subject to quite a few number of limits, models for such scenarios already exist [31]. They are not only phenomenologically consistent, but they also allow for large effects in a vast array of experiments [32,33]. In contrast, in heavy mediator models the constraints from the charged lepton sector lead-in general-to effective couplings whose effects barely exceed few percent [34].
We allow for neutrino vector and axial currents, while for quarks we only consider vector interactions (axial quark currents are spin suppressed), and we assume that all couplings are complex at the renormalizable level. The Lagrangian of the new physics can then be written according to we have dropped lepton flavor indices and we restrict the sum to first generation quarks. In terms of the "fundamental" parameters the nuclear vector current coupling reads (with explicit dependence on the transferred momentum q) where N = A − Z, with A and Z the mass and atomic number of the corresponding nuclide. F n,p (q 2 ) are the neutron and proton nuclear form factors obtained from the Fourier transform of the nucleonic density distributions (in the first Born approximation). Note that this differentiation is particularly relevant for nuclides with N > Z, such as sodium, argon or germanium [20]. The interactions in (1) affect CEνNS processes, as they introduce a q dependence, absent in the SM, that changes the recoil energy spectrum and can either enhance or deplete the expected number of events. Here we will consider both monoand multi-target detectors, and so we write the CEνNS cross section for the i th isotope: Here m i refers to the isotope's atomic mass and ν /m i , E ν being the energy of the incoming neutrino. The overall energy-dependent factor ξ V (q 2 i ) encodes the CP violating physics and reads with g V (q 2 ) the SM contribution weighted properly by the nuclear form factors, namely with g u V = 1/2 − 4/3 sin 2 θ W and g d V = −1/2 + 2/3 sin 2 θ W . For the weak mixing angle we use the central value obtained using the MS renormalization scheme and evaluated at the Z boson mass, sin 2 θ W = 0.23122 [35].
Typical nuclear form factors parametrizations depend on two parameters which are constrained via the corresponding nucleonic density distribution root-mean-square (rms) radii. For a large range of nuclides, proton rms radii have been precisely extracted from a variety of experiments [36]. Consequently, uncertainties on F p (q 2 ) are to a large degree negligible. In contrast, neutron rms radii are poorly known and so uncertainties on F n (q 2 ) can be large. These uncertainties have been recently studied in [20] by assuming that r n rms ⊂ [r p rms , r p rms + 0.3 fm] (for heavy nuclei). The lower bound is well justified in nuclides with N > Z, while the upper one is limited by constraints from neutron skin thickness [37]. In our analysis we choose to fix r n rms = r p rms and use the same form factor parametrization (Helm form factor [38]) for both, neutrons and protons [20]. Doing so, the q 2 dependence of the parameter in (4) comes entirely from the denominator in the second term and that enables a simplification of the multiparameter problem. Note that we do not consider form factor uncertainties in order to avoid mixing their effects with the CP violating effects we want to highlight.
In general the analysis of CP violating effects is a nine parameter problem: the vector boson mass, four moduli and four CP phases. However, the problem can be reduced to three parameters by rewriting the product of the nuclear and neutrino complex couplings in the second term in (4) in terms of real and complex components. A moduli |H V | 2 = Re (H V ) 2 + i Im (H V ) 2 a phase tan φ = Im(H V )/Re(H V ) and the vector boson mass. In terms of the fundamental couplings and CP phases, they are given by . Proceeding in this way the cross section then depends on m V , |H V | and φ through the parameter ξ V in (4), that is now simplified to One can see that the cross section is invariant under φ → −φ, so the analysis can be done by considering φ ⊂ [0, π]. The phase reflection invariance of the cross section assures that the results obtained for such interval hold as well for φ ⊂ [−π, 0]. The boundaries of this interval define the two CP conserving cases of our analysis. Since g V is always negative, φ = 0 always produces destructive interference between the SM and the light vector contribution. At the recoil spectrum level this translates into a depletion of the SM prediction in a certain recoil energy interval. In contrast, φ = π implies always constructive interference, and so an enhancement of the recoil spectrum above the SM expectation. It becomes clear as well that the conclusions derived in terms of |H V | and φ can then be mapped into the eight-dimensional parameter space spanned by the set

III. EVENT RATES, CONSTRAINTS AND PARAMETER SPACE ANALYSIS
To characterize CP violating effects we consider CEνNS produced by fixed target experiments, in particular at CO-HERENT. Qualitatively, the results derived here apply as well in the case of CEνNS induced by reactor and solar ( 8 B) neutrinos. We start the analysis by studying the effects in monotarget sodium ( 23 Na) 2 and argon ( 40 Ar) detectors and then consider the case of a multi-target germanium detector. For the latter case one has to bear in mind that germanium has five stable isotopes 70 Ge, 72 Ge, 73 Ge, 74 Ge and 76 Ge with relative abundances 20.4%, 27.3%, 7.76%, 36.7% and 7.83%, respectively.
In the multi-target case the contribution of the i th isotope to the energy recoil spectrum can be written according to [20] where m det is the detector mass in kg, m = ∑ k X k m k with m k the k th isotope molar mass measured in kg/mol, X i is the isotope relative natural abundance, N A = 6.022 × 10 23 mol −1 , Φ(E ν ) the neutrino flux and F 2 H (q 2 i ) stands for the Helm form factor. The integration limits are E max ν = m µ /2 (for a fixed-target experiment like COHERENT) and E min ν = m i E r /2. The full recoil spectrum then results from dR/dE r = ∑ i dR i /dE r . Note that (8) reduces to the single target case when X i = 1 and m = m k = 0.932A k GeV/c 2 . The number of events in a particular detector is then calculated as with A(E r ) the acceptance function of the experiment. In our analyses we take ∆E r = 1.5 keV.

A. Constraints on light vector mediators
Before proceeding with our analysis it is worth reviewing the constraints to which the light vector mediators we consider are subject to. These constraints arise from beam dump and fixed target experiments, e + e − colliders and LHC, lepton precision experiments, neutrino data as well as astrophysical observations [39]. From the collision of an electron or proton beam on a fixed target, V can be produced either through Bremsstrahlung or meson production and subsequent decay, π 0 → γ + V . The interactions in (1) do not involve charged leptons, hence in the light mediator scenario here considered the coupling of V to electrons is loop suppressed. Limits from electron beam dump and fixed target experiments can be therefore safely ignored. Limits from proton beams are seemingly more relevant since the production of V is possible by Bremsstrahlung-through the vertexpγ µ pV µ -or by meson decay. However, since these searches are based on V decay modes involving charged leptons, again the constraints are weaken by loop suppression factors.
The potential limits from e + e − collider searches (e.g. KLOE, BaBar or Belle-II [40][41][42]), from muon and tau rare decays (SINDRUM and CLEO [43,44]) and from LHC searches (LHCb, ATLAS and CMS [45,46]) are feeble due to the same argument, couplings of V to charged leptons are loop suppressed. As to the limits from neutrino scattering experiments, Borexino, neutrino trident production and TEXONO [10,47,48] involve couplings to charged leptons and so are weak too. Thus, from laboratory experiments the only relevant limit arises from COHERENT CsI phase [1], which have been studied in detail in ref. [23] under the assumption of real parameters. We thus update those limits by considering φ = 0. To do so we follow the same strategy adopted in ref. The bounds include the real cases φ = 0 and φ = π as well as φ = π/3, value for which the limit is found to be the less stringent. [28]. First of all, we define the following spectral χ 2 function where the binning runs over number of photoelectrons n PE (∆n PE = 2 and n PE = 1.17(E r /keV)), α and β are nuisance parameters, σ i are experimental statistical uncertainties and σ α = 0.28 and σ β = 0.25 quantify standard deviations in signal and background respectively. For the calculation of N BSM i we employ eqs. (8) and (9) adapted to include the Cs and I contributions, i.e. m det = 14.6 kg, m → m CsI (m CsI the CsI molar mass) and X i → A i /(A Cs + A I ). For neutrino fluxes we use the following spectral functions normalized according to N = r × n POT /4/π/L 2 , with r = 0.08, n POT = 1.76 × 10 23 and L = 19.3 m. The result is displayed in fig. 1 where it can be seen that the inclusion of CP phases relaxes the bound. We found that the less stringent limit is obtained for φ = π/3, which is about a factor 2.5 larger than the bound obtained at φ = 0. The last limits which apply in our case are of astrophysical origin. Particularly important are horizontal branch stars which have a burning helium core with T 10 8 K 10 −2 MeV. In such an environment vector bosons with masses of up to 10 −1 MeV (from the tail of the thermal distribution) can be produced through Compton scattering processes γ + 4 He → V + 4 He which lead to energy loss. Consistency with the observed number ratio of horizontal branch stars in globular clusters leads to a constraint on the vector-nucleon couplings h p,n V 4 × 10 −11 [49,50]. Assuming h p V = h n V this bound can be translated into |H V | = √ 2Ah n V 6 × 10 −11 A. Relevant as well are the bounds derived from supernova, which exclude regions in parameter space for light vector boson masses up to ∼ 100 MeV 3 . Neutrinos are trapped in the supernova core, so they can only escape by diffusion. Consistency with observations implies t diff ∼ 10 s, therefore limits can be derived by requiring that the new interaction does not sizably disrupt t diff . Further limits can be derived from energy-loss arguments if the new interactions open new channels for neutrino emission, which is the case in the scenario we are considering through V →νν (a process that resemble the plasma process γ →νν). All these limits have been recently reviewed for dark photons in [52] and span a region of parameter space that covers several orders of magnitude in both |H V | and m V .
There are various considerations that have to be taken into account regarding these bounds. First of all, uncertainties on the behavior of core-collapse supernovae are still substantial [53]. As a result, limits from supernovae should be understood as order-of-magnitude estimations. The bounds from stellar cooling arguments discussed above neglect plasma mixing effects, which are relevant whenever the vector has an effective in-medium mixing with the photon. Taking into account these effects, the production rate of the new vectors in the stellar environment is affected, resulting in rather different bounds [54]. Additional environmental effects can alter the bounds from stellar cooling as well as from supernova. This is the case when the vector couples to a scalar which condensates inside macroscopic objects, and screens the charge which V couples to [55,56]. The vector mass in this scenario is proportional to the medium mass density ρ, and so in stellar and supernova environments (high-density environments) its production is no longer possible. In summary, astrophysical constraints should be considered with care as they largely depend on the assumptions used. Thus, for concreteness and because this is the window where new CP violating effects are more pronounced, we focus our analysis in the region m V ⊂ [1, 100] MeV.

B. Parameter space slicing
For CP conserving parameters a full cancellation of the SM contribution, at a given recoil energy, becomes possible in the case φ = 0. In contrast, CP violating parameters do not allow such a possibility. For N events such a cancellation leads to a dip at the recoil energy at which the cancellation takes place. Thus, such a feature in the spectrum will favor CP conserving new physics. Taking this into account, we then split the m V − |H V | plane in two "slices": One for which the recoil spectrum will always exhibit a dip, and a second one for which this is never the case, regardless of φ. The boundary of such regions is clearly determined by the condition that the parameter in eq. (7) vanishes, which translates into a relation between |H V | and m V for a fixed recoil energy, namely In a mono-target experiment the cancellation is exact at a given energy, but in a multi-target detector this is clearly not the case. However, as we will later show in sec. IV A the cancellation is still good enough so to be used to distinguish the CP conserving case from the CP violating one. One can see as well that the position of the dips implied by eq. (12) depends on the type of isotope considered, so different nuclides span different portions of parameter space. This can be seen in fig. 2 in which the parameter space regions m V − |H V | are displayed for 23 Na, 40 Ar and 74 Ge. The regions labeled with COHERENT refer to the energy regions of interest in each case. In all three cases the upper energy isocontour is fixed as E r = 50 keV (determined by the ν e flux kinematic endpoint), and the lower isocontour according to the projected detector recoil energy thresholds. For the NaI detector we assume E th r = 15 keV, for the LAr E th r = 20 keV and for germanium E th r = 2 keV. The lower isocontour at E r = 0 keV defines the boundary of the regions with distinctive and not overlapping CP violating features: dips and degeneracies. The upper isocontour at E r = 100 keV is fixed by the condition of keeping the elastic neutrino-nucleus scattering coherent. Apart from these particular energy isocontours, any other one within the dip zone determines the position of the dip. This means that if future data will show a dip in the event spectrum, and one interprets such a dip in terms of a light vector mediator scenario, its energy location will provide valuable information about the new physics parameters.
To emphasize this observation we consider the 23 Na monotarget detector as well as the germanium multi-target detector. In the first case, we consider the parameter space point {m V , |H V |} = {12 MeV, 1.32 × 10 −7 } as indicated in the left panel of fig. 2 with a black point. That point is located along the E r = 31 keV dotted isocontour, so with φ = 0 a dip in that position is found as shown in the upper left graph in fig. 3 (detector parameters used for this calculation can be seen in tab. I). Data from that detector will identify its exact location up to bin size (energy resolution). Assuming ∆E r = 1.5 keV, such a spectrum will allow to determine |H V | with a 4% accuracy within the range [1.22 × 10 −7 , 1.04 × 10 −6 ] obtained at m V = 1 MeV and m V = 100 MeV, respectively.
As the upper left panel in fig. 3 shows, the presence of CP violating phases produces departures from the dip and so-in principle-one can relate the amount of CP violation to the dip depth. In a mono-target detector this behavior is rather clear given that the dip is related with a cancellation in a single isotope. In a multi-target detector such as for germanium this is not entirely clear. So let us discuss this in more detail. The event rate spectrum is obtained from five different contributions, according to eq. (8). Cancellation at a certain recoil energy for a specific isotope requires a precise value of H V determined by the isotope mass and mass number, and so one expects the remaining contributions not to cancel at that energy.
To investigate what happens in this case, we take the parameter space point {m V , |H V |} = {15 MeV, 4.17 × 10 −7 }, located along the E r = 7 keV isocontour for 74 Ge, as indicated in the right graph in fig. 2 with the black point. For that point, the quantity σ i = X i (dσ i /dE r ) F 2 H (q i ) exactly cancels for 74 Ge and E ν = 50 MeV (any other value allowed by the kinematic criterion E ν > m i E r /2 will lead to the same conclusion). For the remaining isotopes, instead, the following values are found which certainly are rather sizable. The key observation here is that for the same parameter space point all five isotopes generate a dip within a recoil energy interval of 2 keV. More precisely, at E r = 8.4 keV, E r = 7.6 keV, E r = 7.3 keV, E r = 6.4 keV for 70 Ge, 72 Ge, 73 Ge, 76 Ge respectively. Thus, given the spread of those dips, the event rate spectrum does involve a rather pronounced depletion that looks like the dip found in a mono-target detector. Note that the reason behind the appearance of multiple dips from different germanium isotopes has to do with their similarity. The value of |H V | for a fixed vector boson mass is entirely determined by m i and A i through eq. (12). Once the value of |H V | is fixed using the mass and mass number of a particular isotope (in this particular case 74 Ge), eq. (12) fixes as well the points at which the remaining dips will appear. The different recoil energy positions differ only by the relative values of g i V and m i compared to those of the isotope that has been used to fix |H V |. For 70 Ge these differences are order 10% and 5%, while for 76 Ge they are 5% and 2%. Since the differences for 70 Ge are the largest, for this isotope one finds the largest shift from E r = 7 keV. Moreover, since the differences in all cases are small, the spread of the dips is small as well. This conclusion is therefore independent of the parameter space point chosen: There exists as well a dip zone in a multi-target detector (in this case, Germanium based), for which given a point in it the event rate spectrum will always exhibit a dip.
This behavior can be seen in the upper right graph in fig.  3. The overall dip is a result of the five contributions and of their dips spreading over a small recoil energy window around ∼ 7 keV. One can see as well that the presence of CP violating phases has the same effect that in a mono-target detector. As soon as they are switched on, departures from the dip are seen, and the behavior is such that large φ tends to soften the dip. At this point it is therefore clear that in both, mono-and multitarget detectors one could expect a dip which provides information about whether the new vector boson physics involves CP violating phases and-eventually-allows to extract information about its size. We have stressed that in a mono-target detector the exact position of the dip allows for the reconstruction of the coupling |H V |, within an interval. The small spread of the dips for the different germanium isotopes allows the same reconstruction procedure in the multi-target case. An observation of a dip in the event rate spectrum will fix the value of |H V | within an energy recoil isocontour up to the recoil energy resolution, in the NaI, Ge and LAr detectors.
We now turn to the discussion of the "no-dip zone" regions in the graphs in fig. 2. For that purpose we use the LAr detector (middle graph and detector parameters according to tab. I).
As we have already mentioned, the observation of a dip places the possible parameters responsible for a signal within the upper triangles in the graphs in fig. 2 fig. 3. The value for |H V | is obtained by fixing m V = 50 MeV in eq. (7) at E r = 0 keV. In general, for a point in either the boundary of the two regions or in the lower triangle the resulting spectra are rather different from the SM prediction. However, we find that for suitable values of φ one can always find SM+vector spectra that degenerate to a large degree with that of the SM, as illustrated in the graph for φ = 5π/12 and φ = 10π/27. Thus, we conclude that the observation of a SM-like signal cannot be used to rule out CP violating interactions.
We then fix a spectrum generated with real parameters with the point {m V , |H V |} = {16 MeV, 4.45 × 10 −8 } and φ = π. As in the previous case we try to find spectra that degenerate with this one. For the point {50 MeV, 4.25 × 10 −7 } (used in the case of SM degeneracy as well), we find that φ = π/2 and φ = 20π/43 generate spectra that follow rather closely the "real spectrum". In summary, therefore, in the no-dip zone we find that the presence of CP violation leads to degeneracies that call for the inclusion of CP violating effects if CEνNS data is to be interpreted in terms of light vector mediators.

IV. DETERMINING THE SIZE OF CP VIOLATING EFFECTS
We have shown that the inclusion of CP violation has three main effects: (i) suppression of eventual dips in the event rate spectrum, (ii) degeneracy between the SM prediction and the Right graph: Same as in the left graph but for the multi-target germanium detector. In this case the constraints on φ, although still rather competitive, are less pronounced that in the NaI detector due to differences in the detector volume size. The black points indicate the best fit point value.
light vector mediator signal (SM degeneracy), (iii) degeneracy between spectra generated with real parameters and spectra including CP violating phases (real-vs-complex degeneracy).
In what follows we study these three cases in more detail. We do so by taking four data sets that we treat as pseudoexperiments. With them we then perform a χ 2 analysis to show how much φ can be constrained with experimental data. We assume a Poissonian distribution for the binned statistical uncertainty, and so we do not include any steady-state nor beam-on backgrounds.

A. The case of sodium and germanium detectors
To show the degree at which the presence of a dip can constrain the values of φ, we do a counting experiment and perform a χ 2 analysis. For that we employ eq. (10) considering only the signal nuisance parameter and experimental signal uncertainty σ α , which we keep as in the COHERENT CsI phase. In both cases we use the neutrino fluxes from eq. (11) and we fix the remaining parameters according to tab. I. For the NaI detector we use H(E r /keV − 15), while for the germanium detector H(E r /keV − 2). The binning is done in such a way that the first data point is centered at E th r /keV + 1.5. For the NaI analysis, the data points used for N exp are obtained by fixing φ = 0 and the parameter space point shown in the left graph of fig. 2 (black point), with coordinates {12 MeV, 1.32 × 10 7 }. As we mentioned in the previous section, that point generates a dip at E r = 31 keV. We then generated a set of spectra by varying m V within [1, 100] MeV and φ within [−π, π], for the same |H V |. The results of the χ 2 analysis are displayed in the left graph in fig. 4, which shows the 1σ, 2σ and 3σ CL isocontours in the m V − φ. From this graph it can be seen that an observation of a dip in the event spectrum in the NaI detector cannot rule out CP violating interactions, but can place tight bounds on φ. For this particular analysis, all values of φ but those in the range [−π/60, π/60] are excluded at the 1σ level, and increasing the CL does not substantially enlarge the allowed values. For the germanium detector we use as well the point used in the previous section (black point in the left graph in fig. 2 located at {15 MeV, 4.17 × 10 −7 }) to generate N exp . The result of the χ 2 test is shown in the right graph in fig. 4. In this case, the constraints on φ are as well competitive enough but are less tight that those found in the NaI case. They are about a factor ∼ 2 less stringent due to the difference in statistics. As the upper right and left histograms in fig. 3 show, the number of events in the NaI detector is way larger that in the germanium one. As a consequence the statistical uncertainties in NaI are less relevant that in Ge. Regardless of whether one includes or not the background, which increases the statistical uncertainty, this is a rather generic conclusion. The larger the detector the larger the range over which φ can be excluded.

B. The case of the LAr detector
For the LAr detector we assume the parameters shown in tab. I and take for the acceptance function a Heaviside function H(E r /20keV − 20). We proceed basically in the same way that in the sodium and germanium detectors. For the SM degeneracy case N exp is fixed with the SM prediction, while for the real-vs-complex degeneracy case the pseudo-experiment data set is generated fixing φ to π, |H V | to 4.45 × 10 −7 and m V = 16 MeV. For the χ 2 analysis we fix |H V | to 4.25 × 10 −7 and let both m V and φ vary.
The results for both analyses are shown in fig. 5. The left graph shows the 1σ, 2σ and 3σ CL regions for which degeneracy with the SM prediction is induced by complex parameters. The right graph shows the same exclusion regions for which complex parameters mimic an event rate spectrum involving only real parameters. As we have already stressed these re- sults should not be understood as what the actual experiments (or at least simulated data) will achieve, but they do demonstrate our point: Regions in parameter space exist in which CP violating phases can mimic signals that at first sight can be interpreted as either SM-like or entirely generated by real parameters. This analysis therefore allows to establish one of our main points, that is a fully meaningful interpretation of CEνNS data in terms of light vector mediators should come along with the inclusion of CP violating phases.

V. CONCLUSIONS
We have considered the effects of CP violating parameters on CEνNS processes, and for that aim we have considered light vector mediator scenarios. First of all we have introduced a parametrization that reduces the-in principle-nine parameter problem to a three parameter problem. We have demonstrated that this parametrization proves to be extremely useful when dealing with CP violating effects. In contrast to light scalar mediator schemes, light vector mediators allow for interference between the SM and the new physics, something that we have shown enables the splitting of the parameter space into two non-overlapping sectors in which CP violating effects have different manifestations: (i) A region where full destructive interference between the SM and the new vector contribution leads to a dip in the event rate spectrum at a certain recoil energy, (ii) a region where CP violating parameters lead to degeneracies with either the SM prediction or with event rate spectra generated with real parameters.
We have shown that in case (i) information on the amount of CP violation can be obtained. A dip in the event rate spectrum will certainly not allow ruling out CP violation, but will allow to place-in general-stringent constraints on the CP violating effects, with the constraints being more pronounced with larger detector volume. We have pointed out that the dip will as well provide information on the real effective coupling |H V | responsible for the signal, it will enable its reconstruction with a 4% accuracy within an interval spanning about one order of magnitude. In case (ii) we have shown that fairly large regions in parameter space exist where CP violating parameters can mimic CP conserving signals (SM or signals originating from real parameters). We thus stress that meaningful and more sensitive interpretations of future CEνNS data in terms of light vector mediators should include CP violating parameters.
Finally, we point out that the results discussed here apply as well for CEνNS induced by reactor or solar/atmospheric neutrinos. Analyses of CEνNS data from these sources should include as well CP violating effects.