Exploring Light Sterile Neutrinos at Long Baseline Experiments: A Review

: Several anomalies observed in short-baseline neutrino experiments suggest the existence of new light sterile neutrino species. In this review, we describe the potential role of long-baseline experiments in the searches of sterile neutrino properties and, in particular, the new CP-violation phases that appear in the enlarged 3 + 1 scheme. We also assess the impact of light sterile states on the discovery potential of long-baseline experiments of important targets such as the standard 3-ﬂavor CP violation, the neutrino mass hierarchy, and the octant of θ 23


Introduction
More than twenty years ago, groundbreaking observations of neutrinos produced in natural sources (sun and Earth atmosphere) provided the first evidence of neutrino oscillations and established the massive nature of neutrinos [1][2][3][4][5]. Subsequently, the neutrino properties have been clarified by experiments using man-made sources of neutrinos (nuclear reactors and accelerators). The two simple 2-flavor descriptions adopted in the beginning to describe disjointly the solar and the atmospheric neutrino problems have been gradually recognized as two pieces of a single picture, which is presently considered as the standard framework of neutrino oscillations. We recall that in the 3-flavor scheme there are three mass eigenstates ν i with masses m i (i = 1,2,3) [and therefore two independent mass-squared splittings (∆m 2 31 , ∆m 2 21 )], three mixing angles θ 12 , θ 23 , θ 13 , and one CP-phase δ. The neutrino mass hierarchy (NMH) is defined to be normal (NH) if m 3 > m 1,2 or inverted (IH) if m 3 < m 1,2 .
The two standard mass-squared splittings ∆m 2 21 ≡ m 2 2 − m 2 1 and ∆m 2 31 ≡ m 2 3 − m 2 1 are too small to give rise to detectable effects in SBL setups. Therefore, one new much bigger mass-squared difference O(eV 2 ) must be invoked to explain the SBL anomalies. The new hypothetical mass eigenstate must be supposed to be sterile, i.e., a singlet of the standard model gauge group. Several new and more sensitive SBL experiments are underway to put under test such an intriguing hypothesis (see the review in [39]), which, if confirmed would provide a concrete evidence of physics beyond the standard model. In the minimal extension, the so-called 3 + 1 scheme, only one sterile species is introduced. In this scenario, one assumes the existence of one mass eigenstate ν 4 weakly mixed with the active neutrino flavors (ν e , ν µ , ν τ ) and separated from the standard mass eigenstates (ν 1 , ν 2 , ν 3 ) by a O(eV 2 ) difference. In the 3 + 1 framework, there are six mixing angles and three (Dirac) CP-violating phases. Therefore, in the eventuality of a discovery of a light sterile species, we would face the daunting task of nailing down six new properties (three mixing angles, two CP-phases, and the mass-squared splitting ∆m 2 41 ). Several global analyses performed in the 3 + 1 scheme [12][13][14][15] show that the fit noticeably improves with respect to the standard 3-flavor case. However, all such analyses evidence an internal tension between different classes of experiments. More specifically, a tension among the joint disappearance data (ν e → ν e and ν µ → ν µ ) and the appearance data (ν µ → ν e ) is present and has become stronger in the latest analyses. This has led to increasingly lower values for the best fit of θ 14 and especially θ 24 , which currently are close [13] to θ 14 = 8 • and θ 24 = 7 • , and are slightly smaller than the values that we have taken as a benchmark in this review (θ 14 = θ 24 = 9 • ).
The 3 + 1 scenario naturally implies sizeable effects at short distances, where the oscillation factor ∆ 41 ≡ ∆m 2 41 L/4E (L being the baseline and E the neutrino energy) is of order one, and the typical L/E dependency of the signal is expected. However, we stress that sterile neutrinos can leave imprints also in other (non-short-baseline) kinds of experiments, where they have an impact in a more subtle way. In the atmospheric neutrinos, as first shown in [40], at O(TeV) energies, a novel Mikheyev-Smirnov-Wolfenstein (MSW) resonance arises, which produces sizeable modifications of the zenith angle distribution. In the solar sector, a non-zero mixing of the electron neutrino with ν 4 (parameterized by the matrix element U e4 ) leads to detectable deviations from the unitarity of the (ν 1 , ν 2 , ν 3 ) subsystem [36,37] (see also [38]).
Light sterile neutrinos can produce observable effects also in the long-baseline (LBL) accelerator experiments. We recall that such setups, when working in the ν µ → ν e (andν µ →ν e ) appearance channel, are able to identify the 3-flavor CP violation (CPV) induced by the standard CP-phase δ. This sensitivity is strictly related to the circumstance that at long distances the ν µ → ν e conversion probability contains an interference term (which is unobservable at SBL experiments) among the oscillations induced by the solar mass-squared difference and those driven by the atmospheric one. As first shown in [41], if sterile neutrinos participate in the oscillations, a new interference term arises in the conversion probability, which contains one additional CP-phase. Notably, the new genuine 4-flavor interference term is expected to have an amplitude similar to that of the standard 3-flavor interference term. Hence, the detection of the new interference term opens the concrete opportunity to explore the enlarged CPV sector implied by the presence of sterile neutrino species. It should be stressed that, in both the 3-flavor and 4-flavor frameworks, the CP-phases cannot be detected in SBL experiments, since in these setups the two standard frequencies ∆m 2 21 and ∆m 2 31 have a negligible impact. Therefore, the SBL and LBL facilities are synergic in searches of the 3 + 1 framework (and of any other framework that involves more than one sterile state).
These basic observations provide the motivation for writing the present review, in which we discuss the physics potential of the future LBL experiments in the presence of a hypothetical light sterile neutrino. The subject is very active as testified by the numerous works about DUNE [42][43][44][45][46][47][48], T2HK [48][49][50], and T2HKK [48,51]. Other studies on the impact of light sterile neutrinos in LBL setups can be found in [52][53][54][55][56][57][58][59][60]. We underline that, while this review deals with charged current interactions, one can obtain valuable information on active-sterile oscillations parameters also from the analysis of neutral current interactions (see [21][22][23][24] for constraints from existing data and [47,61] for sensitivity studies of future experiments). Finally, we would like to stress that our review is limited to the oscillation phenomenology, although light sterile neutrinos may have an impact also on non-oscillation searches. We mention the studies focused on the leptonic decays of charged leptons and mesons [62], the beta decay [63], and the neutrinoless double-beta decay [64,65].
The review is organized as follows. In Section 2, we present the theoretical framework and introduce the basic formulae for the 4-flavor ν µ → ν e andν µ →ν e transition probabilities. In Section 3, we provide the specifications of the three setups DUNE, T2HK, and ESSνSB, which we use in the numerical simulations. In Section 4, we describe the details of the statistical method that we use for the analysis. In Section 5, we discuss the sensitivity to the LBL experiments to the NMH in the presence of a light sterile neutrino. In Section 6, we describe the sensitivity to CPV and, in Section 7, we study the ability to reconstruct the CP phases. In Section 8, we present an important degeneracy issue, which affects the reconstruction of the octant of θ 23 in the 3 + 1 scheme. We trace the conclusions in Section 9. Appendix A contains the analytical treatment of the matter effects relevant for LBL experiments in the 3 + 1 scheme.
For clearness, we confine the discussion to the case of propagation in vacuum. We address the impact of matter effects in Appendix A. As first shown in [41], the ν µ → ν e transition probability can be written as the sum of three contributions The first term, which is positive-definite, depends on the atmospheric mass-squared splitting and provides the leading contribution to the probability. It takes the form where ∆ ≡ ∆m 2 31 L/4E is the atmospheric oscillating factor, L and E being the neutrino baseline and energy, respectively. The other two contributions in Equation (4) arise from the interference of two different frequencies and are not positive-definite. Specifically, the second term in Equation (4) is related to the interference of the solar and atmospheric frequencies and can be written as P INT I 8s 13 s 12 c 12 s 23 c 23 (α∆) sin ∆ cos(∆ + δ 13 where we introduce the ratio of the solar over the atmospheric mass-squared splitting, α ≡ ∆m 2 21 /∆m 2 31 . We recall that at the first (second) oscillation maximum one has ∆ ∼ π/2 (∆ ∼ 3π/2). The third contribution in Equation (4) appears as a new genuine 4-flavor effect, and is related to the interference of the atmospheric frequency with the new high frequency induced by the presence of the fourth mass eigenstate. This term can be written in the form [41] P INT II 4s 14 s 24 s 13 s 23 sin ∆ sin(∆ + δ 13 − δ 14 ) .
From Equations (5)- (7), we see that the conversion probability depends on (besides the large mixing angle θ 23 ) three small mixing angles: the standard angle θ 13 and two new angles θ 14 and θ 24 . We note that the values of such three mixing angles (estimated in the 3-flavor scenario [66][67][68] for θ 13 , and in the 4-flavor framework [12][13][14][15] for θ 14 and θ 24 ) are similar and one has s 13 ∼ s 14 ∼ s 24 ∼ 0.15 (see Table 1). Therefore, one is naturally induced to consider these three angles as small quantities having the same order of magnitude . We also notice that, since |α| 0.03, it can be considered of order 2 . From inspection of Equations (5)-(7), we derive that the first (leading) contribution is of the second order, while the two interference terms are both of the third order. However, we underline that, differently from the standard interference term in Equation (6), the new sterile-induced interference term in Equation (7) is not proportional to ∆ but to sin ∆; hence, it is not enhanced at the second oscillation maximum. Because of this feature, as our numerical simulations will confirm, the performance of ESSνSB in the 4-flavor scenario is not as good as that of DUNE and T2HK, which work around the first oscillation maximum.
Before closing this section, we underline the fact that the conversion probability in vacuum is independent of the third mixing angle θ 34 and of the related CP-phase δ 34 . As shown in Appendix A, this conclusion does not hold anymore in the presence of matter. In practice, as we discuss in the subsequent sections, the CP-phase δ 34 can be probed only in DUNE, which among the planned LBL experiments, is the most sensitive to the matter effects.

DUNE Setup
Hosted at Fermilab, DUNE is a new-generation long-baseline neutrino oscillation experiment which will play an important role in the future neutrino roadmap to discover the fundamental properties of neutrino [69][70][71][72][73]. DUNE will be composed of three major ingredients: (a) an intense (∼ megawatt), broad-band neutrino beam at Fermilab; (b) a high-precision near neutrino detector just downstream of the neutrino source; and (c) a massive (∼ 40 kt) liquid argon time-projection chamber (LArTPC) far detector hosted deep underground at the Sanford Underground Research Facility (SURF) 1300 km away in Lead, South Dakota. We assume a fiducial mass of 35 kt for the far detector in our simulations, and consider the detector properties which are given in Table 1 of Reference [74]. Concerning the beam, we consider a proton beam power of 708 kW with a proton energy of 120 GeV, which can deliver 6 × 10 20 protons on target on 230 days per calendar year. In our simulation, we have taken the fluxes which were estimated assuming a decay pipe length of 200 m and 200 kA horn current [75]. We consider a total run time of ten years for this experiment, which is equivalent to a total exposure of 248 kt · MW · year. We assume that the DUNE experiment would use half of its full exposure in the neutrino mode, and the remaining half in the antineutrino mode. In our simulations, we take the reconstructed neutrino and anti-neutrino energy range to be 0.5-10 GeV. To incorporate the systematic uncertainties, we consider an uncorrelated 5% normalization error on signal and 5% normalization error on background for both the appearance and disappearance channels to analyze the prospective data from the DUNE experiment. We consider the same set of systematics for both the neutrino and antineutrino channels which are also uncorrelated. For both ν e andν e appearance channels, the backgrounds mostly arise from three different sources: (a) the intrinsic ν e /ν e contamination of the beam; (b) the number of muon events which will be misidentified as electron events; and (c) the neutral current events. Our assumptions on various components of the DUNE set-up are similar to those mentioned in the Conceptual Design Report (CDR) reference design in Reference [70].

T2HK Setup
The main goal of the long-baseline neutrino program at the proposed Hyper-Kamiokande (HK) detector with a neutrino beam from the J-PARC proton synchrotron is to give a conclusive evidence for leptonic CP-violation in neutrino oscillations induced by the CP-phase δ 13 in the 3-flavor neutrino mixing matrix. This setup is commonly known as "T2HK" (Tokai to Hyper-Kamiokande) experiment [76][77][78]. To calculate the physics reach of this setup, we closely follow the experimental specifications as described in References [77,78]. The neutrino beam for HK will be produced at J-PARC from the collision of 30 GeV protons on a graphite target. In our simulations, we consider an integrated proton beam power of 7.5 MW × 10 7 s, which can deliver in total 15.6 × 10 21 protons on target (p.o.t.) with a 30 GeV proton beam. We assume that the T2HK experiment would use 25% of its full exposure in the neutrino mode which is 3.9 × 10 21 p.o.t. and the remaining 75% (11.7 × 10 21 p.o.t.) would be used for the antineutrino run. This ensures that we have nearly equal statistics in both neutrino and antineutrino modes to optimize the search for leptonic CP-violation. These neutrinos and antineutrinos will be observed in the gigantic 560 kt (fiducial) HK water Cherenkov detector in the Tochibora mine, located 8 km south of Super-Kamiokande and 295 km away from J-PARC. The neutrino beamline from J-PARC is designed to produce an off-axis angle of ∼ 2.5 • at the proposed HK site and, therefore, the beam peaks at the first oscillation maximum of 0.6 GeV to enhance the physics sensitivity. This off-axis scheme [79] gives rise to a neutrino beam with a narrow energy spectrum which substantially reduces the intrinsic ν e contamination in the beam and also the background deriving from neutral current events. In our analysis, we consider the reconstructed neutrino and antineutrino energy range of 0.1-1.25 GeV for the appearance channel. In case of disappearance channel, the assumed energy range is 0.1-7 GeV for both the ν µ andν µ candidate events. We match all the signal and background event numbers following Tables 19 and 20 of Reference [77]. The systematic uncertainties play an important role in estimating the physics sensitivity of the T2HK setup. Following Table 21 of Reference [77], we consider an uncorrelated normalization uncertainty of 3.5% for both appearance and disappearance channels in neutrino mode. In the case of antineutrino run, the uncorrelated normalization uncertainties are 6% and 4.5% for appearance and disappearance channels, respectively, and they do not have any correlation with appearance and disappearance channels in neutrino mode. We assume an uncorrelated 10% normalization uncertainty on background for both appearance and disappearance channels in neutrino and antineutrino modes. With all these assumptions on the T2HK setup, we manage to reproduce all the sensitivity results which are given in Reference [77]. Here, we would like to mention that, according to the latest report by the Hyper-Kamiokande Proto-Collaboration [80], the total beam exposure is 27 × 10 21 p.o.t. and the fiducial mass for the proposed HK detector is 374 kt. Comparing the exposures in terms of (kt × p.o.t.), we see that our exposure is 1.156 times smaller than the exposure that has been considered in Reference [80]. However, certainly, the results presented in this work would not change much and the conclusions drawn based on these results would remain valid even if we consider the new exposure as reported in Reference [80].

ESSνSB Setup
ESSνSB is a proposed superbeam on-axis experiment where a very high intense proton beam of energy 2 GeV with an average beam power of 5 MW will be delivered by the European Spallation Source (ESS) linac facility running at 14 Hz. The number of protons on target (POT) per year (208 days) will be 2.7×10 23 [81][82][83][84]. It is worth mentioning here that the future linac upgrade can push the proton energy up to 3.6 GeV. The facility is expected to start taking neutrino data around 2030. We have obtained the fluxes from [85]. They peak around 0.25 GeV. A 500 kt fiducial mass Water Cherenkov detector similar to the properties of the MEMPHYS detector [86,87] is under investigation to explore the neutrino properties in this low energy regime. It has been shown in [81] that, if the detector is placed in any of the existing mines located within 300-600 km from the ESS site at Lund, it will make possible to reach 5σ discovery of leptonic CP-violation with 50% coverage of the whole range of the CP phase. A detailed study on the CP-violation discovery capability of this facility with different baseline and different combinations of neutrino and antineutrino run time has also been performed in [88]. In this review, we consider a baseline of 540 km from Lund to Garpenberg mine located in Sweden and also we have matched the event numbers of Table 3 and all other results given in [81]. At this baseline, it works around the second oscillation maximum and it provides the opportunity to explore the CP-asymmetry, which (in the 3-flavor scheme) is three times larger than the CP-asymmetry at the first oscillation maximum. Although the main disadvantages for going to the second oscillation maximum come from the significant decrease of statistics and cross-sections compared to the first oscillation maximum, the intense beam of this facility compensates those difficulties and makes the statistics competitive to provide interesting results. All our simulations presented here for this setup have been done assuming two years of ν and eight years ofν running. We set the uncorrelated 5% signal normalization and 10% background normalization error for both neutrino and antineutrino appearance and disappearance channels, respectively. For more details of the accelerator facility, beamline design, and detector facility of this setup please, see Reference [81].

Details of the Statistical Analysis
The experimental sensitivities presented in this review are taken form the works [45,50,89]. These have been calculated making use of the GLoBES software [90,91] together with its new physics package. The sterile neutrino effects are included both in the ν µ → ν e appearance channel and in the ν µ → ν µ disappearance channel. The same holds for antineutrino mode. Table 1 displays the true values of the oscillation parameters and their respective ranges of marginalization, which we consider in our numerical simulations. Apart from the atmospheric mixing angle θ 23 , we have fixed the 3-flavor oscillation parameters equal to those obtained in the most recent global fits [66][67][68]. For θ 23 (apart from Section 8), we have set its value to be maximal (45 • ), and in the fit we have marginalized it over the range indicated in Table 1. Concerning the mixing angles that involve the fourth state (θ 14 , θ 24 , and θ 34 ), we have fixed both their true and fit values as given in Table 1. For sin 2 θ 34 , we consider three options, namely 0, 0.025, and 0.25, which are within its current allowed range [12][13][14][15]. Concerning the CP phases δ 14 and δ 34 , we vary their true values in the range [−π, π], and marginalize the fit values in the same range. We set the mass-squared splitting to ∆m 2 41 = 1 eV 2 , which is the value presently indicated by the SBL data. However, we underline that our findings would be unaltered for different values of such a parameter, provided that ∆m 2 41 > 0.1 eV 2 . For such values, the fast oscillations induced by the large mass-squared splitting are totally averaged by the finite energy resolution of the detector. For the same motivation, LBL setups are insensitive to the sign of ∆m 2 41 and this allows us to limit our study to positive values. We have set the line-averaged constant Earth matter density 2 of 2.87 g/cm 3 for all the LBL experiments considered. In our simulations, we have incorporated a full spectral analysis by making use of the binned events spectra for the each LBL experiment. In the statistical analysis, the Poissonian ∆χ 2 has been marginalized over the systematic uncertainties using the pull method as prescribed in References [93,94]. For displaying the results, we show the 1, 2, 3σ confidence levels for 1 d.o.f. adopting the relation Nσ ≡ ∆χ 2 .
In [95], it was shown that the above expression holds in the frequentist method of hypothesis testing. We define the χ 2 function where n is the total number of reconstructed energy bins and Above, N th i ({ω}) represents the theoretical number of CC signal events in the ith energy bin for a set of oscillation parameters ω. N b i ({ω}) denotes the total number of background events 3 . The quantities π s and π b in Equation (9) denote the systematic normalization errors on the signal and background events, respectively. We take the same uncorrelated systematic error for both the neutrino and antineutrino channels. The quantities ξ s and ξ b denote the "pulls" due to the systematic error on the signal and background, respectively. The data in Equation (8) are included through the variable where N ex i is the number of observed CC signal events and N b i is the background as discussed above. To obtain the total χ 2 , we add the χ 2 contributions coming from all the relevant oscillation channels for both neutrino and antineutrino modes in a given experiment In the above expression, we assume that all the oscillation channels for both neutrino and antineutrino modes are uncorrelated, all the energy bins in a given channel are fully correlated, and the systematic errors on signal and background are uncorrelated. The fact that the flux normalization errors in ν µ → ν e and ν µ → ν µ oscillation channels are the same (i.e., they are correlated) is taken into account in the error budget for each of the two channels. However, there are other uncertainties which contribute to the global normalization error for each of the two channels, such as the uncertainties in cross sections, detector efficiencies, etc., which are uncorrelated. For this reason, we simply assume that the total normalization errors in these two channels are uncorrelated. The same holds forν µ →ν e andν µ →ν µ oscillation channels. We think that, with the current understanding of the detectors of DUNE, T2HK, and ESSνSB experiments, it is premature to perform a more accurate analysis taking into account more fine effects as, e.g., the correlation between the flux normalization errors in the appearance and disappearance channels.

Mass Hierarchy Discovery Potential in the 3 + 1 Scheme
In this section, we present the discovery potential of the future LBL experiments to the neutrino mass hierarchy (NMH). We recall that the NMH discovery potential of a given experiment is proportional to the size of matter effects in that setup. This in turn is related to the energy of the neutrino beam of the experiment. As a result, DUNE is very sensitive to NMH, working at the energy of E = 2.5 GeV; T2HK has intermediate sensitivity since it works at E = 0.6 GeV; and ESSνSB has basically no sensitivity working at E = 0.25 GeV. In the following we show the sensitivity of DUNE and T2HK in the 3-flavor and 4-flavor schemes.
In Figure 1, we present the bi-event plots, in which the two axes report the total number of ν e (x-axis) andν e (y-axis) events 4 . In both panels, the black ellipses represent the 3-flavor case, and are obtained by varying the CP-phase δ 13 in the range [−π, π]. In the 3 + 1 scheme, two CP-phases are present and the bi-event plot becomes a blob. In both panels, we assume θ 14 = θ 24 = 9 • , and θ 34 = 0, varying the two phases δ 13 and δ 14 in the range [−π, π]. The 4-flavor full regions can be regarded as a convolution of an ensemble of ellipses with different orientations or, alternatively, as a dense scatter plot resulting from the simultaneous variation of the CP-phases δ 13 and δ 14 . One can see that, in the left panel concerning DUNE, there is a neat separation between the 3-flavor ellipses. This guarantees and exceptional sensitivity of DUNE to the NMH in the standard 3-flavor scheme. In the 3 + 1 scenario, the separation among the blobs corresponding to the two hierarchies is reduced in comparison to the 3-flavor ellipses, but still the two hierarchies remain distinct. Therefore, we expect that the NMH discovery potential will be reduced in the 3 + 1 scheme, but it will not be completely erased. In the right panel, we present the same kind of plot concerning T2HK. In this case, already at the level of the 3-flavor scenario we expect a low sensitivity to NMH since the NH and IH ellipses overlap. In the 3 + 1 scheme, the level of overlapping remains similar.
In Figure 2, we display the discovery potential of the correct hierarchy as a function of the true value of δ 13 considering NH as the true choice. The left (right) panel refers to DUNE (T2HK). In each panel, we provide the results for the 3-flavor case, which is represented by a black curve. In both panels, for the 4-flavor scenario, we have taken θ 14 = θ 24 = 9 • and θ 34 = 0, both true and fit values. Concerning DUNE (left), we present the results for four values of the true δ 14 (−90 • , 90 • , 0 • , and 180 • ) while we marginalize the fit value of δ 14 in the range of [−π, π]. Qualitatively, the shape of the 3 + 1 curves seems similar to the 3-flavor one. In particular, a maximum is present around δ 13 ∼ −90 • , and a minimum around δ 13 ∼ 90 • . It is evident that overall, there is a deterioration of the sensitivity of DUNE for all values of the new CP-phase δ 14 . However, even in the region around the minimum, the sensitivity never decreases below the 5σ level. In the right panel of Figure 2, we plot the NMH discovery potential for T2HK. In the 3-flavor case, on the basis of the bivents plot, one would expect that for some values of the phase δ 13 , the sensitivity should drop to zero. However, quite surprisingly, a non-zero sensitivity appears. As extensively discussed in [50], the sensitivity is due to the energy spectral information. The green band in the right panel represents the T2HK sensitivity in the 3 + 1 scheme. The width of the band is due to the spanning of the true value of δ 14 of the range of [−π, π]. We notice that the shape of the 3 + 1 band is similar to that of the 3-flavor scenario, and, as expected from the bi-event plot, there is only a weak degradation of the NMH discovery potential. In addition, in this case, the binned spectrum has a key role in the NMH discrimination. We can conclude that, albeit the NMH sensitivity of T2HK is quite limited, it is robust with respect to the modifications produced by a light sterile neutrino state.   13 . In both panels, we have fixed true and test θ 14 = θ 24 = 9 • and θ 34 = 0. In both panels, the black curve represents the 3-flavor case. For DUNE (left), in the 3 + 1 scheme, we provide the curves for four different values of true δ 14 marginalizing over test δ 14 . For T2HK (right), the green band is obtained by varying the true value of δ 14 in the range [−π, π] and marginalizing the test value of δ 14 in the same range. Figures taken from [45] (left) and [50] (right).

CP-violation Discovery Potential
The sensitivity of CPV induced by a given (true) value of a CP phase δ true ij is defined as the statistical significance at which one can exclude the test hypothesis of no CPV, i.e., the (test) cases δ test ij = 0 and δ test ij = π. In Figure 3, we report the discovery potential of CPV induced by δ 13 for DUNE (left), T2HK (middle), and ESSνSB (right). We have assumed that the hierarchy is known a priori and is NH. In all panels, the black dashed curve corresponds to the 3-flavor scenario while the colored band represents the 3 + 1 scheme. In the 3 + 1 scenario, we fix the true and test values of θ 14 and θ 24 to be 9 • . In all panels, the colored bands are obtained by varying the unknown true value of δ 14 in the range of [−π, π] while marginalizing over its test value in the same range. We can observe that in all cases, in the 3 + 1 scheme, there is a non-negligible deterioration of the sensitivity. The deterioration is more pronounced in ESSνSB (right). As explained in detail in [89], this different behavior is related to the fact that ESSνSB (in the configuration which we are considering, corresponding to a baseline of 540 km) works at the second oscillation maximum, in contrast to DUNE and T2HK which work around the first oscillation maximum. In the 3 + 1 scheme, one expects that CPV may arise also from the two new phases δ 14 and δ 34 . However, a non-zero sensitivity to δ 34 , can be obtained only in DUNE, where matter effects are noticeable, and for relatively big values of the mixing angle θ 34 . For this reason, we first show the discovery potential of the two experiments T2HK and ESSνSB, which are only sensitive to δ 14 . In the left and right panels of Figure 4, we display the discovery potential of the CPV induced by δ 14 in T2HK and ESSνSB, respectively. We observe that the T2HK performance is much better than that of ESSνSB. In the first case one can reach a sensitivity of 5σ, while in the second one the sensitivity never exceeds the 2σ level.  Figure 4. Discovery potential of the CPV induced by δ 14 for T2HK (left) and ESSνSB (right), assuming the NMH is known to be the NH. We fix the true and test values of θ 14 = θ 24 = 9 • , and we take the true and test θ 34 to be 0 • . In both panels, the colored bands are obtained in the 3 + 1 scheme by varying the unknown true δ 14 in its entire range of [−π, π] in the data while marginalizing over test δ 14 in the same range. Figures taken from [50] (left) and [89] (right).
We think that it is useful to further comment on this huge difference in the sensitivity to CPV induced by δ 14 between the two experiments ESSνSB and T2HK. We notice (see Figure 3) that in the 3-flavor framework both experiments have comparable sensitivities to CPV driven by δ 13 , having both the highest sensitivity of about 8σ for δ 13 ±90 • . This is possible, because, despite the lower statistcal power, ESSνSB takes advantage of the amplification factor proportional to the atmospheric oscillating factor ∆, which appears in the standard 3-flavor interference term [see Equation (6)] of the conversion probability. In fact, this is approximately three times bigger around the second oscillation maximum with respect to the first one. In contrast, in the 3 + 1 scheme, the sensitivity is much worse in ESSνSB. In fact, one can observe that: (i) The degradation of the discovery potential to the CPV induced by δ 13 when going from the 3-flavor to the 3 + 1 framework is much more noticeable in ESSνSB than in T2HK. Taking the values δ 13 = ±90 • as a benchmark (where the highest sensitivity is reached), we find for T2HK only a weak deterioration of the discovery potential from 8σ to 7σ (see middle panel in Figure 3). In ESSνSB, we find instead a pronounced reduction from 8σ to 4.5σ (see right panel in Figure 3); (ii) The sensitivity to the CPV driven by the new CP phase δ 14 is much lower in ESSνSB than in T2HK (2σ vs. 5σ for δ 14 = ±90 • ). The explanation of such a different performance in the 3 + 1 scheme of the two experiments can be understood noticing the fact that ESSνSB works at the second oscillation maximum. As already stressed in Section 2, the new interference term (which is sensitive to δ 14 ) depends on sin ∆ [see Equation (6)], and at the second oscillation maximum it is not amplified by the factor ∆ as happens for the standard 3-flavor interference term (which is sensitive to δ 13 ). In addition, as underlined in [50], T2HK can benefit from the energy spectral information, which plays a crucial role in maintaining a good performance in the 3 + 1 scheme. Indeed, in [50], it was demonstrated that, even if there is a degeneracy at the level of the event counting, the energy spectrum is able to break such a degeneracy, thus boosting the sensitivity. In ESSνSB, the impact of the spectral information is drastically reduced because the energy range at the second oscillation maximum is very narrow and the low statistics impedes to use the information contained in the spectrum. Therefore, we conclude that ESSνSB is not particularly suited for the searches of CPV induced by the presence of sterile neutrinos. We underline that such a conclusion holds for a baseline of 540 km, for which ESSνSB works around the second oscillation maximum. Things may improve by choosing a smaller baseline of 360 or 200 km. In this last case, ESSνSB would work around the first oscillation maximum. Now, let us come to the sensitivity or DUNE to the new CP-phases, which is depicted in Figure 5. In the first panel, for comparison, we display the sensitivity to CPV induced by the standard CP-phase δ 13 . The thinner (magenta) bands represent to the case in which all the three new mixing angles have the same values θ 14 = θ 24 = θ 34 = 9 • . The thicker (green) bands correspond to the case in which θ 14 = θ 24 = 9 • , and θ 34 = 30 • . In each panel, the bands have been obtained by varying the true values of the two undisplayed CP-phases in their allowed ranges of [−π, π] in the data while marginalizing over their fit values in the same range. The comparison of the three panels show that, if all the three mixing angles have the same value θ 14 = θ 24 = θ 34 = 9 • , there is a clear hierarchy in the sensitivity to the three CP-phases. The CP phase δ 13 comes first, δ 14 comes next, and δ 34 is the last one, inducing negligible CPV. Concerning the CP-phase δ 14 (middle), the sensitivity spans over a wide band. In favorable cases, the signal lies above the 3σ level. On the other hand, the lower border of the band is always below the ∼ 2σ. This means that there is not a guaranteed discovery potential at the 3σ confidence level for CPV induced by δ 14 . Finally, coming to the third CP-phase δ 34 (right), we observe that, if the mixing angle θ 34 is big, the sensitivity can be noticeable. In addition, we see that the shape of the band is different from that obtained for the other two CP-phases. This different behavior can be explained by observing that, in this case, the ν µ → ν µ channel also contributes to the overall sensitivity. In fact, it is well known that the ν µ survival probability has a good sensitivity to the NSI-like coupling ε µτ . From the expression of the Hamiltonian in Equation (A13), one can observe that the new mixing angles mimic a NSI-like perturbation ε µτ = rs 24s * 34 , thus a sensitivity of the ν µ survival probability to the CP-phase δ 34 is expected.

Reconstruction of the CP Phases
Until now, we have considered the discovery potential to the CPV induced by the two CP phases δ 13 and δ 14 . Here, we study the capability of the LBL setups to reconstruct the true value of the two CP phases. With this purpose, we consider the four benchmark cases shown in Figure 6. In each panel, we show the region reconstructed by each of the three LBL experiments, DUNE, T2HK, and ESSνSB, around a pair of true values of the two CP-phases δ 13 and δ 14 . The first two panels represent the CP-conserving cases (0, 0) and (π, π). The lower panels concern two CP-violating scenarios (−π/2, −π/2) and (π/2, π/2). In each panel, we show the regions reconstructed around the true values of the two CP phases. In these plots, we have fixed the NH as the true and test hierarchy.
The contours are displayed for the 3σ level (1 d.o.f.) 5 . The performance of ESSνSB in reconstructing δ 13 is similar to that of DUNE and T2HK. In contrast, the reconstruction of δ 14 is better in T2HK and DUNE.
The LBL experiments offer a unique opportunity to identify the θ 23 octant. In fact, a well-known synergy between the ν µ → ν e appearance and ν µ → ν µ disappearance channels [123,126] confers a high sensitivity to the θ 23 octant. The ν µ → ν µ survival probability depends on sin 2 2θ 23 . Then, it is sensitive to deviations from maximal θ 23 but is not sensitive at all to its octant. In contrast, the ν µ → ν e probability is proportional to sin 2 θ 23 and is sensitive to the octant. Therefore, the two channels give complementary information on θ 23 . Notably, the sensitivity can be maximized with a balanced exposure of neutrino and antineutrino runs [128].
Several sensitivity studies to the octant of θ 23 have been performed within the 3-flavor scenario (see [128,[132][133][134][135][136]). In the work [46], the issue has been studied in the 3 + 1 scheme, evidencing for the first time an important degeneracy problem taking DUNE as a case study. We refer the reader to work [46] for analytical details, showing here the numerical results. In a nutshell, the newly identified interference term in Equation (7) that appears in the ν µ → ν e transition probability in Equation (4) can mimic an inversion of the θ 23 octant. As a consequence, for unlucky combinations of the two CP-phases δ 13 and δ 14 , in the 3 + 1 scheme, the discovery potential of the octant of θ 23 is completely lost. The bi-event plot in Figure 7 provides a bird-eye view of what happens. In the 3 + 1 scheme, the theoretical prediction is represented by a colored blob, and the separation among LO and HO is lost. Figure 7. Bi-event plot for the DUNE setup. The ellipses display the 3-flavor scenario, while the colored blobs correspond to the 3 + 1 framework. We take sin 2 θ 23 = 0.42 (0.58) as a representative value for the LO (HO). In the 3-flavor ellipses, the running parameter is δ 13 in the range [−π, π]. In the 3 + 1 blobs, there are two running CP phases, δ 13 and δ 14 . In the 4-flavor case, we have assumed θ 14 = θ 24 = 9 • and θ 34 = 0 • . Figure taken from [46]. 6 As shown in [102,103], in 4 flavors, the condition θ 23 45 • implies an approximate realization of µ ↔ τ symmetry, similar to what occurs in the standard 3-flavor scenario. Therefore, discovering that θ 23 is maximal (non-maximal) would imply that µ ↔ τ symmetry is unbroken (broken), independently of the existence of a light sterile neutrino. Figure 8 shows the DUNE discovery potential for nailing down the true octant as a function of true δ 13 . The left (right) panel refers to the true choice LO-NH (HO-NH). In both panels, we show also the results for the 3-flavor case (black curve). Regarding the 3 + 1 scheme, we show the curves for four benchmark values of true δ 14 (0 • , 180 • , −90 • , 90 • ). In the 3ν framework, the marginalization is performed over (θ 23 , δ 13 ) (test). In the 3 + 1 scenario, we fix θ 14 = θ 24 = 9 • and θ 34 = 0, and marginalize over (θ 23 , δ 13 , δ 14 ) (test). In all cases, we marginalize over the NMH. Figure 8 clearly depicts that in the 3 + 1 scheme there exist unlucky combinations of δ 13 (true) and δ 14 (true) for which the octant sensitivity drops below the 2σ level. We have also verified that for such combinations the energy spectra corresponding to the two octants are almost identical for neutrinos and antineutrinos. Therefore, even a broad-band experiment such as DUNE is not able to resolve the degeneracy introduced by a light sterile neutrino. Very recently, in [48], it has been shown that the situation may improve in T2HKK. However, a direct comparison with our results is not possible because in [48] the benchmark values assumed for the true mixing angles θ 14 , θ 24 , and θ 34 are different (sensibly smaller) than those used in the present review.

Conclusions
Several anomalies observed in short-baseline neutrino experiments suggest the existence of new light sterile neutrino species. In this review, we discuss the potential role of long-baseline experiments in the searches of sterile neutrino properties and, in particular, the new CP-violation phases that appear in the enlarged 3 + 1 scheme. We also assess the impact of light sterile states on the discovery potential of long-baseline experiments of important targets such as the standard 3-flavor CP violation, the neutrino mass hierarchy, and the octant of θ 23 . In the case of the discovery of sterile neutrinos, the planned LBL experiments will have a huge potential to explore the sterile neutrino properties and they will be complementary to SBL experiments.

Acknowledgments:
We are grateful to three anonymous reviewers for the excellent feedback we received.

Conflicts of Interest:
The author declares no conflict of interest.

Appendix A. Conversion Probability in Matter
In matter, the Hamiltonian can be expressed, in the flavor basis, as follows with K denoting the diagonal matrix of the wave numbers where k i1 = ∆m 2 i1 /2E (i = 2, 3, 4) and V is the matrix describing the matter potential where is the charged-current interaction potential of the electron neutrinos in a background of electrons having number density N e , and is the neutral-current interaction potential (equal for all the active neutrino species), where the background neutrons have number density N n . We also introduce the positive-definite ratio which, in the Earth crust, is given by r 0.5. With the purpose of simplifying the treatment of matter effects, we introduce the new basisν =Ū † ν , is the part of the mixing matrix defined in Equation (1), which incorporates only the rotations involving the fourth mass eigenstate. Therefore, the mixing matrix U can be split as follows where U 3ν is the 4 × 4 matrix containing the standard 3-flavor mixing matrix in the (1,2,3) sub-block. In the new basis, the Hamiltonian has the expression where the first term is the kinematic term describing the oscillations in vacuum and the second one is the nonstandard dynamical term. As shown in [41] (see the Appendix therein), since |k 41 | is much larger than one and much larger than |k 21 | and |k 31 |, one can reduce the dynamics to an effective 3-flavor one. Indeed, from Equation (A10), one can see that the (4,4) element ofH is much larger than all the other entries and the fourth eigenvalue ofH is much bigger than the other three ones. As a consequence, the stateν s evolves independent of the others. Extracting the submatrix with indices (1, 2, 3) fromH, one arrives at the 3 × 3 Hamiltonian governing the (ν e ,ν µ ,ν τ ) system, whose dynamical part has the form [41] H where we indicate with † the complex conjugate of the element with the same two indices inverted. Equation (A13) shows that, if the sterile neutrino angles are zero (θ 14 = θ 24 = θ 34 = 0), one recovers the (diagonal) standard 3-flavor MSW Hamiltonian. In general, in the 3 + 1 scenario, the Hamiltonian in Equation (A13) implies both diagonal and off-diagonal corrections. We can observe that these perturbations are formally equivalent to non-standard neutrino interactions (NSI) 7 This formal analogy is useful to interpret the sensitivity to the new dynamical effects implied by 3 + 1 scheme. We recall that, in the ν µ → ν e channel, the NSI that play the most pronounced impact are ε eµ and ε eτ , while in the ν µ → ν µ channel ε µτ has the largest effect. If the three new mixing angles have the same size s 2 14 = s 2 24 = s 2 34 = 0.025, all the perturbations in Equation (A14) are very small (|ε αβ | 0.01) and they have an unobservable impact. In such a case, the dynamics is basically identical to that of the standard 3-flavor scenario. On the other hand, if one allows the third mixing angle to take bigger values (θ 34 ∼ 30 • ), the entries of the third column of the Hamiltonian in Equation (A14) can be noticeably bigger (|ε eτ | |ε µτ | 0.04 and |ε ττ | 0.13). In this last case, one may expect a sizeable effect of ε eτ ≡ rs 14s * 34 in the ν µ → ν e probability, and of ε µτ ≡ rs 24s * 34 in the ν µ → ν µ probability. As a result, one expects that both channels should be sensitive to the third CP-phase δ 34 sinces * 34 ≡ s 34 e iδ 34 . Therefore, differently from the vacuum case, in matter, the flavor transitions are sensitive to θ 34 and the related CP-phase δ 34 . The dependence of both channels from these parameters represents a very peculiar feature, because, in lucky circumstances (i.e., a large value of θ 34 ), the LBL setups are sensitive not only to the two CP-phases δ 13 and δ 14 , but also to δ 34 . Hence, the searches performed at LBL experiments (DUNE in particular) may provide access to the entire CPV sector implied by the 3 + 1 scheme. 7 We stress that this should be taken only as formal analogy. In fact, the real NSI are mediated by heavy particles. In contrast, in the case of sterile neutrinos, there is no heavy mediator and the NSI-like structure of the Hamiltonian is connected to the circumstance that we are working in the new basis introduced in Equation (A7), which is rotated with respect to the original flavor basis. We mention that a similar analogy has been noticed in the field of solar neutrino conversion in the presence of sterile states [36].