Light sterile neutrino sensitivity of 163 Ho experiments

,


Introduction
The observation of neutrino oscillations is a clear demonstration that neutrinos are massive particles. The data of solar, atmospheric and long-baseline neutrino oscillation experiments are explained in the standard scheme of three-neutrino mixing (3ν) in which the three active neutrinos ν e , ν µ , ν τ are unitary linear combinations of the three massive neutrinos ν 1 , ν 2 , ν 3 , with respective masses m 1 , m 2 , m 3 (see refs. [1,2]). A global analysis of the data of solar, atmospheric and long-baseline neutrino oscillation experiments [3][4][5] leads to an accurate determination of the three mixing angles and of the two independent solar and atmospheric squared-mass differences, ∆m 2 SOL = ∆m 2 21 7.4 × 10 −5 eV 2 and ∆m 2 ATM = |∆m 2 31 | |∆m 2 32 | 2.50 × 10 −3 eV 2 [5], with ∆m 2 kj ≡ m 2 k − m 2 j . The 3ν paradigm is presently challenged by anomalies found in short-baseline (SBL) neutrino oscillation experiments: the reactor antineutrino anomaly [6][7][8], which is a deficit of the rate ofν e events measured in reactor neutrino experiments; the Gallium neutrino anomaly [9][10][11][12][13], consisting in a deficit of the rate of ν e events measured in the Gallium radioactive source experiments GALLEX [14] and SAGE [15]; the LSND anomaly, which is an excess of the rate ofν e events in a beam composed mainly ofν µ 's produced by µ + decay at rest [16,17]. These anomalies cannot be explained by neutrino oscillations in the 3ν scenario. A possible explanation, still in the framework of neutrino oscillations, requires the existence of a new short-baseline squared-mass difference ∆m 2 SBL 1 eV 2 , which is much larger than the solar and atmospheric squared-mass differences. The new short-baseline squared-mass difference requires the existence of at least one new massive neutrino ν 4 with mass m 4 such that ∆m 2 SBL = |∆m 2 41 | (see the review in ref. [18]). In the flavor basis there must be a sterile neutrino ν s and the mixing of the left-handed neutrino fields is given by U αk ν kL (α = e, µ, τ, s), (1.1)
Although the data of short-baseline experiments can be explained either with m 1 , m 2 , m 3 < m 4 or m 4 < m 1 , m 2 , m 3 , the second case is strongly disfavored by cosmological measurements [80] and by the experimental bounds on neutrinoless double-β decay (assuming that massive neutrinos are Majorana particles; see ref. [81]), which favor a scenario with m 1 , m 2 , m 3 m 4 . In this paper we consider this scenario, which implies that m 2 4 ∆m 2 41 = ∆m 2 SBL 1 eV. This relation allows us to compare the results of the experiments measuring directly m 4 with the results of short-baseline neutrino oscillation experiments.
The fact that a heavy massive neutrino ν 4 is mixing with the three light massive neutrinos to compose the electron neutrino can give a very clear fingerprint in the spectra of nuclear beta decay and electron capture. This means that experiments designed for the direct investigation of the electron (anti-)neutrino mass have the possibility to scrutinize the parameter space of active-sterile neutrino mixing indicated by short-baseline experiments. The evidence for the existence of such a sterile neutrino would be a kink in the spectrum positioned at Q − m 4 [82][83][84], where Q is the energy available to the decay, which is given by the difference between the masses of the parent and daughter atoms. The amplitude of this kink is related to the mixing |U e4 | that ν 4 has with ν e .
Presently there are two nuclides which are used for the direct investigation of neutrino masses: 1 tritium ( 3 H) undergoing the beta-decay process 3 H → 3 He + e − +ν e and holmium ( 163 Ho) undergoing the electron-capture process e − + 163 Ho → 163 Dy + ν e (see the reviews in refs. [85][86][87]). New generation experiments using these nuclides are expected to reach a sensitivity to sub-eV values of the effective electron neutrino mass. Therefore they can JHEP06(2016)061 investigate the existence of an eV-scale massive neutrino which has a significant mixing with ν e . The sensitivity that can be reached by the KATRIN experiment [88,89] to the signature of ν 4 in the 3 H beta spectrum was studied in refs. [89][90][91][92][93]. These works proved that the KATRIN experiment could, within three years of measuring time and at nominal performance, rule out a large part of the parameters space required to explain the anomalies in short-baseline experiments.
In this paper we investigate the sensitivity of 163 Ho electron capture experiments to neutrino masses in the standard framework of three-neutrino mixing and in the framework of 3+1 neutrino mixing with an eV-scale sterile neutrino. We consider in particular the first two planned phases of the ECHo project, ECHo-1k and ECHo-1M [94,95]. Other 163 Ho experimental projects are HOLMES [96], which has a program to investigate small neutrino masses competitive with the ECHo program, and NuMECS [97], which at least for the moment is only aiming at a precise measurement of the 163 Ho decay spectrum.
The plan of the paper is as follows. In section 2 we describe the effect of neutrino masses in 163 Ho electron capture. In section 3 we describe the characteristics of the ECHo experiment which are relevant for our analysis. In section 4 we present our estimation of the sensitivity of the ECHo experiment to the effective neutrino mass in the 3ν framework. In section 5 we calculate the sensitivity of the ECHo experiment to m 4 in the case of 3+1 neutrino mixing and we compare it with the region in the space of the mixing parameters allowed by the global analysis of short-baseline neutrino oscillation data. In section 6 we present our conclusions.

163 Ho electron capture process
The property that makes 163 Ho the best isotope for investigating the electron neutrino mass is the very small energy Q available to the decay. Recently, the Q-value has been precisely determined by Penning trap mass spectrometry to be Q = 2833 ± 30 stat ± 15 syst eV [98]. At the present knowledge, this is the lowest Q for all nuclides undergoing electron capture processes.
In an electron capture process one electron from the 163 Ho atomic levels is captured, leading to a transformation of a proton into a neutron and the emission of an electron neutrino. The daughter atom, 163 Dy is left in an excited state which, at the leading order, is described by a hole in the shell from which the electron has been captured and one electron more in the 4f shell with respect to the ones foreseen for the dysprosium atom in the ground state. The excitation energy can then be released through the emission of x-rays or electrons (Auger or Coster-Kronig transition). We indicate the sum of all the energy released in the electron capture process minus the one taken away by the neutrino as E c . This is the quantity that is measured by calorimetric techniques in modern experiments studying the 163 Ho decay [99]. The concept of these experiments was initially proposed more then thirty year ago by De Rujula and Lusignoli [100,101].
The decay scheme can then be divided in the following two steps:

JHEP06(2016)061
Considering only first order transitions and neglecting the nuclear recoil, the expected spectrum for the excitation energy is characterized by a sum of Breit-Wigner resonances modulated by the phase space factor (see refs. [85][86][87]): Here, P i is the probability of electron capture from the i-shell, which has been calculated in ref. [102] using a fully relativistic approach. It is given by is the square of single electron wave functions of the parent atom at the nuclear radius R and B i is a correction for electron exchange and overlap. The energy E i is the peak energy of the i-th resonance, which is given in a first approximation by the difference between the binding energy in the daughter atom of the electron that has been captured and the binding energy of the 4f electron: The width Γ i is the intrinsic width of the resonance, which is related to the half-life of the excited i-state. The Heaviside function Θ(Q − E c − m k ) ensures the reality of the expression. The parameters describing the atomic excited states are taken from ref. [102] and listed in table 1.
The fraction of the calorimetrically measured spectrum which is mostly affected by finite neutrino masses is the endpoint region, where the emitted neutrino has only a few eV of kinetic energy. In the following, we consider a detector with energy resolution of 5 or 2 eV and we assume that the masses m 1 , m 2 , m 3 of the three massive neutrinos ν 1 , ν 2 , ν 3 , in the framework of the standard three-neutrino mixing scenario, are much smaller than the energy resolution. In this case, eq. (2.3) can be approximated by with the effective electron neutrino mass This approximation is consistent with the most stringent upper limits on m ν found in the Mainz [103] and Troitsk [104] experiments: at 95% CL.

The ECHo experiment
The ECHo experiment is designed to reach a sub-eV sensitivity to the electron neutrino mass through the analysis of the endpoint region of the 163 Ho spectrum. The concept at the basis of this experiment is that all the energy released during the 163 Ho electron JHEP06(2016)061 capture, besides that taken away by the neutrino, is measured with high precision. Large arrays of low temperature metallic magnetic calorimeters (MMCs) [105] will be used. The 163 Ho atoms will be completely enclosed in the energy absorber, which consists of a gold film with about 10 µm thickness and a 200 × 200 µm 2 surface area. Such an absorber is thermally coupled to a temperature sensor, which is a thin film of a paramagnetic material, typically gold doped with a few hundreds ppm of erbium, sitting in an external stable magnetic field. The sensor is then weakly coupled to the thermal bath kept at a constant temperature of less then 30 mK. When energy is deposited in the detector, its temperature increases leading to a change of magnetization of the sensor which is read out as a change of flux by low-noise high-bandwidth dc-SQUIDs (Superconducting QUantum Interference Devices). An energy resolution as good as 1.6 eV FWHM at 6 keV has already been achieved with MMCs developed for soft x-ray spectroscopy as well as very precise calibration functions [106]. An intrinsic background is the unresolved pileup which is related to the finite time resolution of the detector and to the fact that, since the 163 Ho is enclosed in the detector itself, each 163 Ho decay leads to a signal. Therefore, two or more events which occur in a time interval shorter than the risetime of the pulse are misidentified as a single event with an energy given approximately by the sum of the single event energies. The fraction of pileup events is given by the product of the activity in the detector and the risetime of the signal. In order to be able to investigate small neutrino masses, the unresolved pileup fraction f pp should be smaller than 10 −5 . The first prototypes of MMCs with embedded 163 Ho have already shown a risetime of the order of 100 ns [107], which allows for single pixel activities of the order of a few tens of Bq. The goal of the ECHo experiment is to have the sum of all other background contributions in the endpoint region of the spectrum at least one order of magnitude smaller than the unresolved pileup. This corresponds to a background parameter b < 5 × 10 −5 counts/eV/det/day. During the first phase of the ECHo experiment, ECHo-1k, which already started, more then 10 10 events of 163 Ho electron capture will be collected in one year of measuring time by having a 163 Ho source of the order of 1000 Bq distributed into about 100 MMCs. The major goals of this phase are to obtain an energy resolution better than 5 eV FWHM for multiplexed detectors and an unresolved pileup fraction smaller than 10 −5 . Achieving these goals will allow the ECHo Collaboration to reach a limit on the electron neutrino mass below 10 eV, which is more than one order of magnitude better than the current JHEP06(2016)061 limit on the electron neutrino mass obtained with a 163 Ho electron capture experiment, m ν < 225 eV at 95% C.L. [108].
In the second phase of ECHo, called ECHo-1M, a 163 Ho source of the order of 1 MBq will be embedded in a large number of pixels divided into multiplexed arrays. The aim of this phase is to measure a 163 Ho spectrum with about 10 14 events with an energy resolution better that 2 eV FWHM and an unresolved pileup fraction of the order of 10 −6 . With ECHo-1M the sensitivity to the electron neutrino mass will reach the sub-eV region [109].
The discussed sensitivities are based on the analysis of simulated 163 Ho spectra which are generated using only the first order excited states in 163 Dy. Higher order excited states, like the one corresponding to the formation of two holes in the 163 Dy atom after the electron capture, even if they have a much smaller probability to occur, can play a quite important role in the region near the endpoint of the spectrum. The role of higher order excitations has been recently studied in refs. [110][111][112][113]. There is still not a good agreement among the different authors on the expected structures in the 163 Ho spectrum due to these excitations. The available data on the 163 Ho spectrum [97,114,115] are still not able to clearly resolve the controversy. An important point to mention is that the two-hole excitations in which an electron is "shaken-off" in the continuum may imply a substantial increase of the fraction of events in the endpoint region of the spectrum [112,113]. Therefore, by presenting limits on the sensitivity based only on the first order excited states, we provide upper values of the sensitivity that could be reached with a well-defined experimental configuration.

3ν mixing
In this section we describe our methodology to obtain the sensitivity for the neutrino mass in the ECHo experiment and we present our results for the sensitivity to m ν in the standard case of three-neutrino mixing. Previous analyses of the sensitivity of 163 Ho experiments with various configurations have been presented in refs. [99,[116][117][118].
The theoretical spectrum of 163 Ho electron capture events as a function of the total released energy E c is given by with the normalized total spectrum Here S EC (E c , m ν ) is the normalized electron-capture spectrum  the measuring time; the background 2 B = bt m ; the fraction of pileup events f pp , that, in a first approximation, is given by f pp = τ R A, where τ R is the time resolution. The detector energy response R ∆E (E c ) is assumed to be Gaussian: with variance relate to the full width at half maximum by the usual relation σ ∆E = ∆E FWHM /2.35. In eqs. (4.1) and (4.2), the symbol ⊗ represents a convolution. The self-convolution of the normalized spectrum in the second term of eq. (4.2) accounts for the pileup effect. In order to speed up the computer-intensive evaluation of the sensitivity to m ν , in this term we used the normalized spectrum S EC (E c , 0), neglecting the small effects due to m ν . Figure 1 illustrates the effect of an effective neutrino mass m ν = 1 eV on the spectrum S EC and on the total spectrum S tot without and with the convolution with the detector energy response R ∆E (E c ) for ∆E FWHM = 2 eV. One can see that in the limit of negligible unresolved pileup, represented by the curves labeled S EC , the difference between the spectra with m ν = 0 and m ν = 1 eV without and with the convolution with the detector energy response is similar. On the other hand, the difference of the total spectra S tot for m ν = 0 and m ν = 1 eV is significantly affected by the energy resolution of the detector. Without considering the finite energy resolution of the detector, the difference between S tot (m ν = 0) and S tot (m ν = 1 eV) is relatively large around Q−m ν , where S EC (m ν = 1 eV) vanishes and only the pileup contributes. Since this difference is strongly reduced by the convolution with the detector energy response, it is clear that the sensitivity to the neutrino mass     statistics. We adopted the Feldman-Cousins definition of sensitivity 3 given in ref. [119]: "the sensitivity is defined as the average upper limit one would get from an ensemble of experiments with the expected background and no true signal." Hence, for a given experimental configuration we generated N sim simulations of the data in the case m ν = 0, for each simulation we found the corresponding upper limit for m ν , and we calculated the sensitivity as the median of these upper limits. We did not use the mean of the upper limits, which may be interpreted as the "average" in the Feldman-Cousins definition of sensitivity, because the mean is not defined in the case of limits on more than one parameter, as in the case of 3+1 neutrino mixing considered in section 5. On the other hand, for N par parameters the median is defined as the N par hypersurface which encloses all the values of the parameters which are allowed by more than 50% of the simulations. 4 We considered two experimental configurations corresponding to the expected performances of the ECHo-1k and ECHo-1M experiments [94,95]. For ECHo-1k we considered ∆E FWHM = 5 eV and N ev = 10 10 , whereas for ECHo-1M we considered ∆E FWHM = 2 eV and N ev = 10 14 . We considered different values of the pileup fraction f pp from 10 −8 to 10 −4 . We also neglected the background B, which in the ECHo experiment is expected to be at least one order of magnitude smaller than the unresolved pileup, as already mentioned above (see also the discussion in ref. [118]).
The simulations have been generated with Q = 2.833 keV and the simulated data have been fitted from E min c = 2.2 keV to E max c = 3.2 keV with different bin sizes. We checked that the results are independent of the bin size as long as it is smaller than the energy resolution uncertainty σ ∆E .

JHEP06(2016)061
The theoretical average number of events in the i th energy bin (with i = 1, . . . , N bins ) is given by where E min i and E max i are, respectively, the lower and upper borders of the bin. In the j th simulation of the data (with j = 1, . . . , N sim ), the number of events (n sim i ) j in the i th bin is obtained with a Poisson fluctuation around the theoretical average number of events n th i (0), corresponding to m ν = 0. The χ 2 of the j th simulation is given by . (4.6) Although specific values of Q, N ev , f pp and B have to be used for the generation of the simulated (n sim i ) j , we do not make any assumption for the values of these parameters in the expression of n th i (m ν ) used in the fit of the simulated data and χ 2 j (m ν ) is calculated by marginalizing over them. This method reflects the probable real experimental approach, in which these parameters will be determined by the data. 5 For each simulation j we compute the upper limit (m UL ν ) j for m ν at CL confidence level using the relation: where (χ 2 j ) min is the minimum of χ 2 j (m ν ) and ∆χ 2 (CL) = 2.71, 4.0, 9.0 for CL = 90%, 95.45%, 99.73%, respectively. As explained above, the sensitivity m sens ν is given by the median of the upper limits (m UL ν ) j in the ensemble of N sim simulations. For the first stage of the ECHo experiment, ECHo-1k, the aim is to achieve a total statistics of N ev 10 10 with an energy resolution ∆E FWHM 5 eV. Figure 2 shows our estimation of the sensitivity to m ν of ECHo-1k as a function of f pp . One can see that for the foreseen value f pp 10 −6 the sensitivity will be around 6.5 (7.9) eV at 2σ (3σ), which will represent an improvement of more than one order of magnitude with respect to the current limit m ν < 225 eV at 2σ [108] obtained with a 163 Ho electron capture experiment. One can also notice that the sensitivity does not improve much decreasing the value of f pp below about 10 −6 . This happens for the following two reasons:  2. The average number of pileup events in an energy interval of the order of the energy resolution ∆E FWHM near the endpoint is smaller than one. Indeed, neglecting the small effects due to the neutrino mass, the average number of pileup events in the energy interval ∆E FWHM is smaller than one for Since near the endpoint we have S EC (E c , 0)⊗S EC (E c , 0) = 4.07×10 −6 , for N ev = 10 10 and ∆E FWHM 5 eV we obtain the condition f pp 5 × 10 −7 .
In the second stage of the ECHo experiment, ECHo-1M, it is expected to have an energy resolution better than ∆E FWHM = 2 eV. Figure 3 shows our estimation of the sensitivity to m ν of ECHo-1M as a function of f pp when the same statistics of N ev = 10 10 expected in the ECHo-1k will be reached. Comparing figures 2 and 3, one can see that the improvement of the energy resolution generates a small improvement of the sensitivity. One can also notice a flatter behavior of the sensitivity for f pp 10 −6 in figure 3 than in figure 2. This is due to the fact that albeit the condition 1 above is satisfied for f pp 1 × 10 −6 , the condition 2 is already satisfied for f pp 1 × 10 −6 . Figure 4 shows our estimation of the final sensitivity to m ν of ECHo-1M as a function of f pp when the statistics of N ev = 10 14 will be reached. One can see that it is possible to reach a sensitivity of about 0.6 (0.7) eV at 2σ (3σ) for the foreseen value f pp 10 −6 . Hence, ECHo-1M will enter into the sub-eV region of m ν , not far from the expected 0.2 eV sensitivity of KATRIN [88,89]. The behavior of the sensitivity for f pp 10 −6 is less flat than those in figure 2 and 3 because only the condition 1 above is satisfied for f pp 1 × 10 −6 , whereas the condition 2 is satisfied only for f pp 1 × 10 −10 . Figure 5 shows our results for the sensitivity to m ν as a function of the total statistics N ev for ∆E FWHM = 2 eV, f pp = 10 −6 and B = 0. One can see that m sens ν follows the expected proportionality to N −1/4 ev explained above, in agreement with the calculations presented in refs. [87,118].

JHEP06(2016)061
In a future experiment larger than ECHo-1M it may be possible to have a total statistics of N ev 10 16 . Figure 5 shows that in this case it will be possible to reach a sensitivity to m ν of about 0.2 eV, similar to that expected for the KATRIN experiment [88,89].

3+1 neutrino mixing
In this section we present our analysis of the sensitivity of future 163 Ho experiments to the effects of the heavy neutrino ν 4 in the 3+1 neutrino mixing scheme considering m 4 m k for k = 1, 2, 3 as explained in the introductory section 1. In this case, eq. (2.3) can be approximated by with m ν given by eq. (2.5). Therefore, the complete spectrum can be described as a sum of two spectra, one ending at Q − m ν with a fraction of events given by (1 − |U 2 e4 |) and the other ending at Q − m 4 with a fraction of events given by |U 2 e4 |. The spectrum in eq. (5.1) depends on the three neutrino parameters m ν , m 4 and |U e4 | 2 and allows to calculate the sensitivity of a 163 Ho in the corresponding three-dimensional parameter space. Here, we simplify the problem by assuming that m ν is much smaller than the sensitivity of the experiment. Hence, we consider the simplified spectrum which depends only on m 4 and |U e4 | 2 . We considered the space of the two parameters ∆m 2 41 m 2 4 and sin 2 2ϑ ee = 4|U e4 | 2 (1− |U e4 | 2 ) in order to compare the sensitivity of 163 Ho experiments with the results of global analyses of short-baseline neutrino oscillation data [18,22,55,[120][121][122][123][124][125][126][127][128][129]. We calculated the sensitivity of 163 Ho experiments in the sin 2 2ϑ ee -∆m 2 41 plane with a method similar to that described in section 4, using the spectrum in eq. (5.2). In the 3+1 case, for each simulation j we compute the allowed region at CL confidence level in the sin 2 2ϑ ee -∆m 2 41 plane using the relation: where (χ 2 j ) min is the minimum of χ 2 j (sin 2 2ϑ ee , ∆m 2 41 ) and ∆χ 2 (CL) = 4.61, 6.18, 11.83 for CL = 90%, 95.45%, 99.73%, respectively. We calculate the region of sensitivity in the sin 2 2ϑ ee -∆m 2 41 plane as the set of points which are not allowed by the inequality (5.3) in at least 50% of the simulations (see the discussion on the definition of sensitivity in section 4).

JHEP06(2016)061
From figure 6 one can see that the sensitivity to ∆m 2 41 worsens decreasing sin 2 2ϑ ee . Indeed, for small values of sin 2 2ϑ ee we have |U e4 | 2 sin 2 2ϑ ee /4 and the contribution of m 2 4 ∆m 2 41 to the spectrum (5.2) is suppressed. On the other hand, the sensitivity to m 2 4 ∆m 2 41 for sin 2 2ϑ ee = 1 is only slightly worse of that for m 2 ν in the three-neutrino mixing case discussed in section 4, because sin 2 2ϑ ee = 1 corresponds to |U e4 | 2 = 1/2.
In figure 6 we also depicted the region allowed at 95.45% C.L. by a global fit of shortbaseline neutrino oscillation data [18,126] and the 95.45% C.L. allowed regions obtained by restricting the analysis to the data of ν e andν e disappearance experiments [13,130], taking into account the Mainz [131] and Troitsk [132,133] bounds. These last regions are interesting because it is possible that the disappearance of ν e andν e indicated by the reactor and Gallium anomalies will be confirmed by the future experiments whereas the LSND anomaly will not.
From figure 6 one can see that the ν e andν e disappearance region is wider than the globally allowed region and extends to values of ∆m 2 41 as large as about 80 eV 2 . Hence, it can be partially explored by the ECHo-1M experiment, which is expected to have a statistics of N ev 10 14 . Figure 6 shows that in order to explore the region which is allowed by the global fit of short-baseline neutrino oscillation data it will be necessary to make a 163 Ho experiment with a statistics N ev 10 16 . One can also see that an 163 Ho experiment with this statistics will be competitive with the KATRIN experiment [89], a result that is consistent with that for the sensitivity on m ν in the standard framework of three-neutrino mixing discussed at the end of section 4. Figure 6 also shows that the exploration of the small-∆m 2 41 regions allowed by the ν e andν e disappearance data will require a statistics as high as N ev ≈ 10 18 .

Conclusions
In this paper we presented the results of an analysis of the sensitivity of 163 Ho experiments to neutrino masses considering first the effective neutrino mass m ν in the standard framework of three-neutrino mixing (see eq. (2.5)) and then an additional mass m 4 at the eV scale in the framework of 3+1 neutrino mixing with a sterile neutrino. We considered the experimental setups corresponding to the two planned stages of the ECHo project, ECHo-1k and ECHo-1M [94,95].
We found that the ECHo-1k experiment can reach a sensitivity to m ν of about 6.5 eV at 2σ with a total statistics of N ev 10 10 , an energy resolution ∆E FWHM 5 eV and a pileup fraction f pp 10 −6 . Although this sensitivity is still not competitive with that of tritium-decay experiments, it will represent an improvement of more than one order of magnitude with respect to the current limit m ν < 225 eV at 2σ [108] obtained with a 163 Ho electron capture experiment. We also found that the ECHo-1k experiment will not allow to put more stringent limits on the mass and mixing of ν 4 than those already obtained in the Mainz [131] and Troitsk [132,133] experiments.
According to our estimation, the second stage of the ECHo project, ECHo-1M, can reach a sensitivity to m ν of about 0.7 eV at 2σ with N ev 10 14 , ∆E FWHM [18,126]. The gray curves enclose the 95.45% C.L. allowed regions obtained by restricting the analysis to the data of ν e andν e disappearance experiments [13,130], taking into account the Mainz [131] and Troitsk [132,133] bounds. Also shown is the expected 95% C.L. sensitivity of the KATRIN experiment [89]. 10 −6 . This result will narrow the gap between the sensitivities of tritium-decay experiments and 163 Ho electron capture experiments. Indeed, 0.7 eV is smaller than the current upper limit of about 2 eV at 2σ obtained in the Mainz [103] and Troitsk [104] experiments and it is not too far from the expected sensitivity of about 0.2 eV of the KATRIN experiment [88,89].
We found that the ECHo-1M experiment will be sensitive to the large-sin 2 2ϑ ee and large-∆m 2 41 part of the region in the sin 2 2ϑ ee -∆m 2 41 plane which is allowed by the data of short-baseline ν e andν e disappearance experiments [13,130], taking into account the Mainz [131] and Troitsk [132,133] bounds. However, it cannot explore the region allowed by the global fit of short-baseline neutrino oscillation data [18,126].
According to our calculations, a 163 Ho electron capture experiment with ∆E FWHM 2 eV and f pp 10 −6 will be competitive with the KATRIN tritium-decay experiment [88,89] by reaching a statistics of N ev ≈ 10 16 . Such an experiment will cover a large part of the region in the sin 2 2ϑ ee -∆m 2 41 plane which is allowed by the data of short-baseline ν e and ν e disappearance experiments and the large-sin 2 2ϑ ee and large-∆m 2 41 part of the region allowed by the global fit of short-baseline neutrino oscillation data.
In order to explore all the region allowed by the global fit of short-baseline neutrino oscillation it will be necessary to have a statistics of N ev ≈ 10 17 and to cover all the region allowed by the data of short-baseline ν e andν e disappearance experiments a statistics of N ev ≈ 10 18 will be needed. These large event numbers seem unreachable now, but we think that we should be optimistic, taking into account that the development of 163 Ho electron capture experiment is only at the beginning.