Coherent NeutrinoNucleus Scattering and New Neutrino Interactions
Abstract
We investigate the potential to probe new neutrino physics with future experiments measuring coherent neutrinonucleus scattering. Experiments with high statistics should become feasible soon and allow to constrain parameters with unprecedented precision. Using a benchmark setup for a future experiment probing reactor neutrinos, we study the sensitivity on neutrino nonstandard interactions and new exotic neutral currents (scalar, tensor, etc). Compared to Fermi interaction, percent and permille level strengths of the new interactions can be probed, superseding for some observables the limits from future neutrino oscillation experiments by up to two orders of magnitude.
I Introduction
Coherent neutrinonucleus scattering (CS) Freedman (1974); Freedman et al. (1977); Drukier and Stodolsky (1984) is a tree level process that is predicted by the Standard Model, but has not yet been observed. While being conceptually highly interesting and allowing measurements of electroweak observables at low momentum transfer, the process is also of phenomenological importance for future dark matter direct detection experiments Billard et al. (2014). Moreover, it holds the potential to probe new neutrino physics Barranco et al. (2005); Dutta et al. (2016, 2015); Papoulias and Kosmas (2015), which is the main focus of this paper.
In CS, low energy neutrinos interact with the protons and neutrons in the nuclei coherently, which significantly enhances the cross section. While large fluxes of neutrinos are available from nuclear research or commercial reactors, the recoil energy of the nuclei is difficult to detect since it is very low. However, prompted partly by developments in dark matter direct detection experiments, modern lowthreshold detectors make the detection of CS technically feasible Scholberg (2006); Wong et al. (2006). Combined with smart shielding techniques, highrate and lowbackground experiments are possible^{1}^{1}1See, for instance, Ref. Akimov et al. (2015); Wong (2015); Kerman et al. (2016); Soma et al. (2016); Anderson et al. (2011) for recent studies.. Future CS experiments may thus provide precision test of neutrino interactions in the Standard Model and strong constraints on new physics related to neutrinos.
In this paper, we will study the sensitivities of CS on possible new neutrino interactions, mainly assuming Germanium detectors with subkeV threshold, detecting reactor antineutrinos. For illustration, we will assume values of the experimental parameters within reach of current technology^{2}^{2}2See e.g. https://indico.mpp.mpg.de/event/3121/session/3/contribution/18/material/slides/0.pdf for details.. To make our study applicable to various new physics models, we will adopt a modelindependent approach, only considering the low energy effective operators of neutrinos and quarks. This includes not only the widelydiscussed conventional NonStandard Interactions (NSI) Davidson et al. (2003) which are in (chiral) vector form, but also more exotic interactions that could be in scalar or tensor form. What distinguishes this paper from previous studies of the potential implications of coherent scattering Barranco et al. (2005); Dutta et al. (2016, 2015); Papoulias and Kosmas (2015); Cerdeno et al. (2016), is the inclusion of such exotic interactions, and a comparative study on how different experimental details (such as energy threshold or neutrino flux uncertainty) influence the sensitivity on new physics.
The paper is organized as follows. We start by introducing CS in the Standard Model in Sec. II. Then we study the effect of new physics on CS, based on effective operators of neutrinos and quarks, which can be divided into two cases, the conventional NSI in Sec. III and exotic neutral currents in Sec. IV. In Sec. V, we consider a benchmark setup for a CS experiment and perform fit on parameters from the Standard Model, NSI and exotic neutral currents to study the sensitivities of such an experiment on them. We conclude in Sec. VI. Details on the calculation of the cross section with both spin0 and spin nuclei are delegated to Appendix A and B. Some useful relations connecting the fundamental coupling constants of exotic neutral currents to the effective parameters in CS are given in Appendix C.
Ii Coherent neutrinonucleus scattering in the Standard Model
ii.1 Cross Section
In the Standard Model (SM), the Neutral Current (NC) interaction enables low energy neutrinos with MeV (corresponding to length scales of m) to interact coherently with protons and neutrons in a nucleus, which significantly enhances the cross section for a large nucleus. For a nucleus at rest with protons and neutrons, the coherent cross section Freedman (1974); Freedman et al. (1977); Papoulias and Kosmas (2015) (see Appendix A) is given by
(1) 
where is defined as
(2) 
Here , , and are the Fermi constant, the Weinberg angle, and the mass of the nucleus, respectively. Since at low energies Erler and RamseyMusolf (2005), we have , which implies that the cross section is dominated by the neutron number; is the form factor of the nucleus and its coherent limit () is . For higher energies, due to loss of coherence, it will be smaller than (for a recent quantitative study, see Ref. Kerman et al. (2016)). The recoil energy of the nucleus has a maximal value , determined by the initial neutrino energy and the nucleus mass :
(3) 
For new physics beyond the SM, both Eq. (1) and Eq. (2) could be modified but Eq. (3) still holds since it is determined purely from relativistic kinematics.
Eq. (2) was derived under the assumption that the nucleus is a spin0 particle Freedman (1974) (see also Appendix A of this paper). However, this is not always true because a nucleus with odd is a fermion, examples are or . In Appendix B, we calculate the simplest nonzero case, spin. It turns out that the difference is small, given by
(4) 
Thus, the only difference is a term proportional to , which is usually negligible in the coherence scattering process. In principle the nucleus could also be some higher spin particle but based on Eq. (4) it is reasonable to deduce that the difference should be suppressed for a large nucleus.
ii.2 Detection
Note that the recoil energy is the only measurable effect of coherent neutrino scattering. Depending on the type of detectors, the method to measure is very different. We will focus here on Germanium detectors which measure the ionization energy , which is a fraction of the deposited recoil energy . The fraction is defined as the quenching factor , typically within 0.15 to 0.3 for subkeV recoil energies (see e.g. Figs. 5 and 7 in Ref. Barker and Mei (2012)). The quenching factor at subkeV energies is not well known due to lack of experimental data. In typical models like the one proposed by Lindhard et al. Lindhard et al. (1963), the recoil energy depends on , so would be a (not necessarily linear) function of . However, no matter what the exact form of the function would be, once is measured, it can be converted to , provided that this function has been theoretically calculated Barker and Mei (2012) or experimentally measured^{3}^{3}3One approach to measure the quenching factor is to use neutron scattering, as performed in the CDEXTEXONO collaboration above keV energies. For more details see https://wwwgerda.mpp.mpg.de/symp/20_Ruan.pdf. In the future subkeV measurements will be performed. . We assume that the quenching factor can be measured precisely in the future, and thus use the recoil energy rather than the ionization energy . All the results in our paper can be simply converted from the dependence to the dependence, provided that the function is determined.
Generally for all types of detectors there is a detection threshold on , denoted as . Therefore, for a given the recoil energy of detected events should be within the range and the measurable reduced total cross section is
(5) 
Due to the threshold , low energy neutrinos are impossible to detect if their energies are lower than
(6) 
For example, if keV Wong (2015) then neutrinos should have MeV in order to be detected in a Ge detector. On the other hand, if we consider reactor neutrinos, the flux decreases exponentially at high energy. Therefore there is a limited range of for detection. To illustrate this, we plot in Fig. 1 the reduced cross section [given by Eq. (5)], a typical reactor neutrino flux and their product , which is essentially proportional to the event rate. As Fig. 1 shows, the product is small at both low (2 MeV) and high (8 MeV) energies.
From the above discussion it is clear that the total event number decreases drastically when the detection threshold is increased. To show this, we compute the total event numbers with different detection thresholds, plotted in Fig. 2, where one can see that the event number drops by 2 orders of magnitude if rises from keV to 0.8 keV. Therefore lowering the detection threshold is very crucial in order to obtain large event numbers. For this plot we have assumed a 100 kg Ge detector located 10 m away from a 1 GW (thermal power) reactor and taking data for five years. For the neutrino flux , we have taken the spectrum from a recent theoretical calculation in Ref. Kopeikin (2012), normalized to (corresponding to 10 m distance from the reactor). Those values will serve as benchmark for our assumed future experiment, and can be used as a definition of our assumed “exposure” of
(7) 
In Fig. 2 we also show the effect of an assumed constant background of 1 cpd and 3 cpd (1 cpd = ). The background may come from various sources, such as the intrinsic radioactivity of the material in the detector, ambient radioactivity near the nuclear reactor or cosmic rays. Estimation of the background is very much involved and depends significantly on the details of the detector. The GEMMA experiment Beda et al. (2013) states a background level of about 2 cpd and the TEXONO collaboration is aiming at developing a Ge detector with a background of 1 cpd Wong et al. (2006). Note however that the mentioned background numbers apply to somewhat different energy scales and different background sources. Taking into account the low background levels that various double beta decay and dark matter direct detection exeriments have reached, plus noting the developements on active shielding at shallow depth Heusser et al. (2015), we estimate that such low background rates can be achieved.
In reality, not only the total event number but also the distribution of events will be measured, giving us a spectrum with respect to the recoil energy . The spectrum provides more information than the total event number. The advantage to exploit the spectrum is that it is not influenced strongly by many uncertainties such as the flux normalization, the distance and fiducial mass of the detector, the form factor, etc. All those effects can be described roughly by an overall factor that enhances/reduces the total event number.
If the events are conservatively counted in many bins, the th bin with width starting from , then the expectation of the event number in the th bin is
(8) 
Here is the number of Ge nuclei^{4}^{4}4Natural Germanium consists of (), (27.45%), (7.76%), (36.52%) and (7.75%). Here we take in average. Note that spindependent axial couplings in the Standard Model lead to smaller coherence factors depending on the spin of the nucleus, not on or as the vector interaction that gives the leading contribution, see Appendix B. This will be a permille effect, see Cerdeno et al. (2016). in the detector and is the running time of detection, taken as 5 years. The neutrino flux has been taken from Kopeikin (2012), and the dimensionless function is defined as [see Eq. (1)]
(9) 
Note that when new physics beyond the SM is involved, one only needs to modify in Eq. (8) and in Eq. (9) according to the new physics. Taking the flux from Ref. Kopeikin (2012) and setting the background at constant 3 cpd, the event numbers computed according to Eq. (8) are presented in Fig. 3 as a function of .
We should mention here that the calculation of the reactor neutrino flux is very complicated. Though a lot of effort was spent to calculate the flux in the literature (see e.g. Kopeikin (2012); Achkar et al. (1996); Schreckenbach et al. (1985); Mention et al. (2011); Huber (2011) and references therein), so far a very precise result is lacking, especially for neutrino energies below 2 MeV where the error could be large as 7%. The best understood range is from 2 MeV to 6 MeV, but still with 3% error. Recently, measurements from the RENO Seo (2015); Choi et al. (2016), Daya Bay An et al. (2016) and Double Chooz Abe et al. (2016) experiments showed disagreement with the theoretical calculation around 5 MeV, the infamous 5 MeV bump. Its observation implies that we might have not fully understood the reactor neutrino flux. A particle physics origin of the bump seems very unlikely. In the next few years, both the theoretical understanding and experimental measurement will be significantly improved Buck et al. (2015); Giunti (2016); Huber (2016) so that the flux will be known more precisely and also the issue of the 5 MeV bump will be resolved once our assumed future CS experiment is running. Anyway, the sensitivities of coherent scattering on new physics depend very little on the presence of the bump. A quantitative study on the influence of the 5 MeV bump is presented below.
Iii NonStandard Interactions in Coherent Scattering
Coherent scattering could provide very strong constraints on neutrino NonStandard Interactions (NSI). Those have been widely studied in the literature but so far the experimental constraints on some of its parameters are still very poor (see the reviews Davidson et al. (2003) and Ohlsson (2013)), especially the couplings of neutrinos to quarks.
In this work, only the neutrinoquark sector of NSI is relevant. The Lagrangian is
(10) 
where are the three flavors of neutrinos, and , are the nonstandard vector and axialvector coupling constants, respectively. Interpreting the NSI terms in analogy to Fermi theory implies that the various are given by
(11) 
i.e. are related to new interactions mediated (for ) by TeVscale particles with mass ( denotes a new coupling constant). In neutrino oscillation experiments longrange forces have a similar effect as matterinduced NSIs Heeck and Rodejohann (2011). We note that such light mediators could strongly affect the shape of the spectrum under study here, and thus distinguish both possibilities.
When the NSI Lagrangian (10) is added to the SM, the CS differential cross section is changed only by an overall factor. For the SM, the differential cross section is given in Eq. (1) which is proportional to given by Eq. (2). For the NSI, following the calculation in Appendix A, it is straightforward to obtain the result, which is simply replacing with , given by
(12) 
Here the modified weak charge is defined as
(13)  
Setting the to zero gives back the result from Eq. (2). The axial vector couplings in Eq. (10) do not appear in Eq. (13) because of parity symmetry being present in large nuclei (see the discussion in Appendix A). The cross section only depends on the vector couplings , which for simplicity will be denoted by henceforth. Even though this removes a lot of parameters, we are still confronted with a sixdimensional parameter space,
(14) 
So far the best constraints Davidson et al. (2003) on () come from CHARM inelastic scattering Dorenbosch et al. (1986). The 3limits are
(15)  
(16)  
(17)  
(18) 
assuming that for each bound only the corresponding coupling is nonzero. As one can see, these bounds are typically of order one. For the flavor, the best constraints are from de Gouvea et al. (2001); Davidson et al. (2003),
(19) 
This bound comes from a 1loop diagram including the four fermion vertex of . As a consequence, the result depends on the scale of the underlying UV complete model (recall that NSI in Eq. (10) are nonrenormalizable). In Ref. Davidson et al. (2003) it is assumed to obtain this bound.
To understand how NSI affect CS, we study the dependence of on the six parameters in Eq. (14) with several plots in Fig. 4. Each plot displays the ratio as a function of two in Eq. (14), while the other four are set to zero. Note that Eq. (13) is symmetric under exchange of and , thus we combine plots for and since for coherent scattering they have the same effect.
From the top two panels in Fig. 4 one can see that there is one direction (the green line) in which is always equal to , approximately at . Under the approximation that one can immediately derive this relation from Eq. (13). It implies that CS does not have any sensitivity on NSI parameters along this direction, which has already been discussed in Refs. Barranco et al. (2005); Scholberg (2006). In the other panels, the direction with also exists but in the form of a curve rather than a straight line. Therefore, degeneracies are present, which in case the NSI actually exist would need to be broken by other experiments, most notably neutrino oscillation experiments.
Fig. 4 also shows that the ratio could significantly deviate from . Even for small values of in the range , could vanish () or rise to twice the SM value (). Therefore once coherent scattering is observed, it will provide a significant constraint on NSI parameters. Besides, among the six plots in Fig. 4, only the top right one does not include , which implies that if the measured cross section is lower than the SM value, then or have to be nonzero in order to explain the deficit by NSI. A statistical analysis of the sensitivity on NSI will be performed in section V.
Iv Exotic Neutral Currents in Coherent Scattering
Apart from the NSI which only couple neutrinos to quarks in (chiral) vector form, more “exotic” new interactions could be present. There are five types of possible interactions, scalar (), pseudoscalar (), vector (), axialvector (), and tensor () interactions:^{5}^{5}5To make the following calculation more compact, we assume that the SM neutral current interaction is included in Eq. (20) rather than adding Eq. (20) to the SM Lagrangian. As a consequence, in the SM and are nonzero.
(20) 
where stands for and quarks and
(21) 
In analogy to Eq. (11), the and are expected to be of order , with new exchange particles and coupling constants . The coefficients and in Eq. (20) are dimensionless and in principle can be complex numbers. However if the interaction term is not selfconjugate, it would be added by its complex conjugate, which is proportional to for and for . Since , and are real numbers, without loss of generality we can take and
(22) 
as real numbers. We will assume for simplicity that and . This still leaves us with 10 free parameters.
A subtle issue related to and should be clarified here. When the tensor is coupled to , there are two possibilities, and . On the other hand, there could be new interactions such as and , which seem not to be included in Eq. (20). But due to the identity
(23) 
all these new possibilities can be transformed into the tensor form appearing in Eq. (20):
(24) 
Since the coherent nature of the scattering requires low energy, we can treat the nucleus in the coherent scattering as a pointlike particle. Depending on the spin of the nucleus, it can be described by a scalar field, a Dirac field or even higher spin fields. As we have shown in Eq. (4), for low energy scattering the difference of treating the nucleus as a spin0 or spin1/2 particle is negligible, and in fact identical to order . In the following calculation we will treat the nucleus as a spin1/2 particle since for automatic calculation implemented by packages (we use both FeynCalc Shtabovenko et al. (2016); Mertig et al. (1991) and PackageX Patel (2015)) it is technically simpler than the scalar treatment. Consequently, the effective Lagrangian of neutrinonucleus interactions has the same form as Eq. (20) with replaced by the Dirac field of the nucleus, i.e.
(25) 
Note that to define the effective couplings of to , here we use which should be related to the more fundamental couplings . Since the relations are lengthy and also involve form factors, we present them in Appendix C. From now on, we will consider and as parameters of interest, and will present results in terms of those. We are not aware of literature limits on the parameters, which would have been obtained from past neutrinonucleon scattering experiments. Since the event numbers in our benchmark experiment are much larger than in such experiments, the sensitivities we will derive later would surely be orders of magnitude better.
From Eq. (25), we can write down the scattering amplitude,
(26) 
Note that for general interactions, the coherent cross sections of and are different [in the SM coherent and cross sections are the same due to the approximate parity symmetry in nuclei, see comments after Eq. (69)]. Since we are studying the coherent scattering of reactor neutrinos, only righthanded antineutrinos are considered. Therefore we have attached a projection to the initial neutrino state , so that the trace technology applies,
(27) 
The result is given by
(28)  
where
(29) 
and
(30) 
As we can see, the cross section only depends on 5 parameters, , compared to the 10 parameters in Eq. (25).
The first three lines of Eq. (28) come from scalar and pseudoscalar, vector and axial vector, and tensor interactions respectively while the term is an interference term of the (pseudo) scalar and tensor interactions. Despite that contains both scalar and pseudoscalar contributions, for simplicity we will refer to as the scalar interaction of neutrinos with nuclei. In the same way, though the vector couplings and the axial vector couplings all appear in , we still call and the vector and axial interactions, respectively.
Comparing Eq. (28) to Eq. (1), we obtain the SM values of these parameters,
(31) 
where the number is computed for Germanium, i.e. by taking , and .
There are some noteworthy comments to make from Eq. (28):

There is no interference term of (axial) vector interactions with other interactions. But the vector interaction interferes with the axial interaction.

The other terms (i.e. scalar, axial, tensor interaction terms and two interference terms) have different energy dependence. If any distortion on the recoil energy spectrum would be observed, then these new interactions could be the explanation.

For vector interactions, is zero at [defined in Eq. (3)] but it could be nonzero if other types of interactions exist. This is shown in Fig. 5 where at the threshold the cross section is seen to be zero (blue curve) for the SM but nonzero (red curve) if other types of exotic neutral currents exist.

Introducing exotic neutral currents (except for vector interactions) can not reduce the cross section since the sum of the other terms besides the term in Eq. (28) is always above zero. So if the observed events are less than the expectation from the SM, one should consider modifications only limited to the vector sector rather than introducing scalar or tensor interactions.
The various modifications we have discussed so far (NSI, exotic neutral currents and the 5 MeV bump) can influence the event numbers. In Fig. 6 we illustrate this for three examples. A feature of NSI is that they could result in a significant deficit (excess is also possible) of the event number, whereas exotic neutral currents only lead to an excess if is fixed at its SM value. In principle exotic neutral currents could also lead to a deficit by lowering , but this is indistinguishable from the NSI case. The 5 MeV bump in the neutrino flux also leads to an excess, but is not very significant. Here we take the size of the 5 MeV bump from a recent fit in Ref. Huber (2016) (given by its Fig. 2). The excess in the 0.100.15 keV bin is only about 1%, which can be easily hidden in the systematic uncertainties. As mentioned before, since other experiments will collect with different reactor types a large amount of event numbers around the 5 MeV bump, it is very likely that before a highly sensitive Ge detector with very small systematic uncertainties is running, the 5 MeV bump problem will be solved (both in theory and experiment).
Another important difference is that the above three cases have very different effects on the distortion of the spectrum. NSI will not lead to any distortion at all since it only changes the overall factor in the differential cross section while the other two cases, exotic neutral currents and the 5 MeV bump, lead to different distortions. In Fig. 7 we show variations of the event ratio as a function of in several situations, where is the event number expected from for the SM and includes new interactions or the 5 MeV bump. For exotic neutral currents, we plot three examples to illustrate the effects from scalar, axial vector and tensor interactions with , and respectively. All the other parameters, if not mentioned, have been set to the SM values given by Eq. (31). As one can see, for exotic neutral currents the ratios increase with but the slopes are different. Scalar interactions would produce the strongest distortion on the spectrum followed by axial vector and then tensor. The 5 MeV bump also generates an increasing ratio with respect to below 0.45 keV. However, the ratio drops down at higher energies and finally reaches 1. The reason is that neutrinos at 5 MeV will only contribute to the events below keV [cf. Eq. (3)]. Thus in the range close to but less than 0.7 keV, the events from the 5 MeV bump should quickly decrease. If all neutrinos in the bump only had energies exactly at 5 MeV, then the contribution should completely vanish above 0.7 keV. However, taking the width of the bump into consideration, the actual limit is a little higher than 0.7 keV.
V Sensitivities from a fit
In this section, we will adopt fit to study the sensitivities of such our assumed future experiment. For convenience, let us state again our assumed exposure of from Eq. (7), corresponding e.g. to a 100 kg Germanium detector running for 5 years, located at a distance of 10 m from a reactor with 1 GW thermal power, normalized to a total flux of . We will assume different thresholds of , or keV, and a constant background of cpd = .
v.1 Statistical Treatment
Because the event number in each bin is very large, and thus almost in a Gaussian distribution, we can take the following function
(32) 
where denotes generally the parameters of interest, e.g. for the NSI case or for exotic neutral currents. The event numbers in each bin as expected in the SM are denoted as . The statistical uncertainty and the systematic uncertainty of the event number in the th bin are given by
(33) 
Here the background is set at 3 cpd (1 cpd = ). We assume that is proportional to the event number with a coefficient . Many systematic uncertainties simply change the total event number without leading to strong distortions of the spectrum, e.g. the uncertainties from the evaluation of the total flux of neutrinos, nuclear fuel supply, detection efficiency, fiducial mass of the detector, distance and geometry corrections, etc. To describe this part of systematic uncertainties, we introduce a normalization factor with a small uncertainty , while the other systematic uncertainties remain in . Of course in a more realistic study one should parametrize specifically the effect of every systematic uncertainty, some of which can not be described by this approach. For the current stage, we simply adopt Eq. (32) for our sensitivity study, which nevertheless should provide realistic results.
It is sometimes useful to know the value of at the minimum of analytically, which is
(34) 
One can use Eq. (34) to marginalize and obtain the function that we are actually interested in,
(35) 
If coherent scattering has been successfully detected, the first task is to compare the measured total cross section with the SM prediction in Eqs. (1) and (2). The ratio indicates any deviation from the SM. One can compute the above function to estimate the sensitivity on this ratio ( in this case simply stands for ). The result is shown in Fig. 8, where we have assumed three different configurations:

conservative configuration: .

intermediate configuration: .

optimistic configuration: .
Even in the conservative configuration, the experiment can measure with good precision, at 3. In the intermediate case, , while for the optimistic case , all at 3. As it turns out, the improvement in sensitivity on new physics parameters between the conservative and intermediate configuration is about a factor of two. Roughly another factor of two can be gained when going from the intermediate configuration to the somewhat overly optimistic one. The choices we made for the various configurations should therefore give a feeling on the final sensitivity of such experiments.
v.2 Low Energy Determination of the Weinberg Angle
The measurement of can also be converted into a measurement of the electroweak angle according to Eq. (2), which would provide important complementary insight into electroweak precision observables at low energies. In Fig. 9 we show the sensitivity of this experiment on , assuming its SM value at low scale of (red line). The blue curves represent 3bounds, solid for a conservative configuration and dashed for a optimistic one . From Fig. 9 we can see that in the conservative configuration is expected to be measured, depending on the threshold, to a good precision between 10% and 20%, while in the optimistic configuration, this would be improved roughly by an order of magnitude. For a threshold of 0.1 keV, the precision at is , or about 1%, to be compared with the dedicated P2 experiment Berger et al. (2015), which aims at a precision of 0.13%.
v.3 NonStandard Interactions
The effect of the conventional NSI, as we have discussed in Sec. III, is merely a correction on the overall factor . The dependence of on various parameters has been studied in Sec. III and was displayed in Fig. 4. We will study here the sensitivities of each individually, assuming that all others are zero. The sensitivities on the NSI parameters in both the conservative and optimistic configurations are presented in Fig. 10. The left panel is for with or . The right panel is for with or , the cases are indistinguishable. The left panel of Fig. 10 shows that the CS experiment in the conservative configuration could constrain to order , much better than the current best bounds given in Eqs. (15) and (16), which are typically of order . If one takes the optimistic configuration, then the constraint would reach the order of . The constraints on and , however, are relatively weaker, about 0.07 to (0.02 to 0.03) for the conservative (optimistic) configuration. This can be easily understood from the form of in Eq. (13). For the channel, this is still a significant improvement compared to the current bound in Eqs. (17) and (18) while for the channel, the current known bound is already very strong [see Eq. (19)]; therefore, even if we take the optimistic estimation, the constraint would not exceed the known bound.
To summarize the comparison discussed above, we plot those bounds in Fig. 11. The blue and dark blue bars shows the 3 bounds from our assumed CS experiment with conservative and optimistic configuration, respectively. The light blue bars represent the best known bounds from the review Davidson et al. (2003), see Eqs. (15) and (19). We also add the expected bounds de Gouvea and Kelly (2016) from the future longbaseline neutrino experiment DUNE in the plot. The sensitivity of DUNE on NSI is based on the modified matter effect of neutrino oscillations caused by NSI parameters. The parameter set constrained by DUNE is actually
(36) 
where is the number density of the corresponding fermion . Their relative density ratio is approximately in the Earth crust. Focusing on one parameter at a time, the limits on from Ref. de Gouvea and Kelly (2016) can be translated into limits on . This serves to compare the sensitivities and is displayed in Fig. 11. Even the conservative configuration improves the bounds on and considerably beyond current limits and future DUNE sensitivities. The limits obtainable in our benchmark experiment are summarized in Table 1.
v.4 Exotic Neutral Currents
Next we shall study the sensitivity on the exotic neutral currents discussed in Sec. IV. The cross section (28) only depends on 5 effective parameters , and we will perform a fit on those. Similar to the NSI analysis, we will focus on one type of exotic interactions at a time. However, in our parametrization is necessarily nonzero as it includes the SM contribution. So each time we take two nonzero parameters in the fit. One is and the other one is from exotic couplings. We also take to zero since nonzero would stem from the interference of scalar and tensor interactions, i.e., would require the coexistence of two new interactions. Therefore we only consider three cases, , , and .
The result is given in Fig. 12 with both the conservative (left panels) and optimistic (right panels) configurations taken. In the conservative configuration, the sensitivity on is correlated with the other parameters. For example, if then would be only allowed to stay in the regime at 99.7% confidence level; if there is a sizable contribution from the tensor interaction with, say, then is allowed to significantly deviate from the SM value, going down to . The correlation could be avoided if the systematic uncertainties and the threshold are improved to the optimistic configuration, as is shown in the right panels of Fig. 12. The qualitative explanation is that for large systematic uncertainties, the sensitivity will mainly depend on the total event number while the constraint from the spectrum information is not significant. In this case the tensor interaction will mimic the vector interaction in the signal, since they both contribute to the total event number. If the systematic uncertainties are small enough so that the spectrum is also measured to good accuracy, then the spectrum information could distinguish the contribution of the tensor interaction from the vector interaction. The same argument also applies for the other two cases and . Therefore in future CS experiments reducing the systematic uncertainties is very important to distinguish signals from new exotic interactions and the SM interaction. The limits obtainable in our benchmark experiment are summarized in Table 2.
Conservative  

Intermediate  
Optimistic 
Vi Conclusion
Future coherent neutrinonucleus scattering experiments will provide exciting new data to test Standard Model and new neutrino physics to unprecedented accuracy. We have assumed here a future experiment with a low threshold (down to 0.1 keV nuclear recoil) Germanium detector, with experimental benchmark numbers of 500 kg years GW reactor neutrinos and a baseline of 10 m. We firmly believe that such a setup is achievable within the next decade, and it will provide event numbers of the order of . Constraints on neutrino nonstandard interactions and exotic neutral current interactions were evaluated. The expected sensitivities were shown to reach percent and permille level when compared to Fermi interaction, significantly better than expected constraints from oscillation experiments. We have demonstrated that such comparably compact coherent scattering experiments open a new window into exciting physics and should be pursued actively.
Acknowledgements.
We thank Carlos Yaguna and Thomas Rink for many useful discussions. WR is supported by the DFG with grant RO 2516/61 in the Heisenberg Programme.Appendix A Cross Section Calculation of coherent Scattering in the Standard Model
In the SM, the neutral current (NC) is
(37)  
(38) 
where stands for all elementary fermions in the SM and are their left/righthanded components,
(39) 
Here are determined by the quantum numbers of the corresponding fermions under :
(40)  