High-spin states of⁹⁵Tc: towards a systematic investigation of $\nu d_{5/2} \rightarrow \nu g_{7/2}$ excitations along $N=52$ isotones

High-spin states in atomic nuclei are generally generated through two distinct mechanisms: the collective mode, associated with the rotation of a deformed nuclear shape, and the non-collective (single-particle) mode, in which angular momentum is generated by the successive alignment of valence nucleons in specific orbitals [1−3]. Although high-jorbitals play a particularly important role in the non-collective mode, medium- and low-jorbitals also contribute significantly to the generation of angular momentum. Nuclei in the $ A\approx90 $ mass region, located near the⁸⁸Sr ( $ Z=38, N=50 $ ) core, are well known to exhibit predominantly single-particle excitations at low and medium spins [4−14]. The low-lying states in nuclei with $ Z \gt 38 $ and $ N \gt 50 $ can be interpreted by coupling protons in the $ \pi (p_{1/2}, g_{9/2}) $ orbitals above the $ Z = 38 $ shell to neutrons in the $ \nu (d_{5/2}, s_{1/2}) $ orbitals above the $ N = 50 $ shell, with⁸⁸Sr treated as an inert core. For states at high energy, three competing excitation mechanisms are involved: proton promotion across the $ Z=38 $ subshell, neutron excitations across the $ N=50 $ closed shell, and neutron excitations through the $ N=56 $ subshell ( $ d_{5/2} \rightarrow g_{7/2} $ excitation). Among these mechanisms, proton excitations across the $ Z=38 $ subshell are energetically favored because of the relatively small $ Z = 38 $ subshell gap [15]. Breaking the $ N=50 $ core through neutron $ g_{9/2}^{-1} $ excitations has been suggested as a mechanism for generating higher angular momentum in several $ N=52 $ isotones, such as⁹⁴Mo [7] and⁹⁶Ru [5]. The excitation energy required to break the $ N=50 $ core increases with proton number, as reported in Refs. [16,17], whereas the energy of the $ \nu g_{7/2} $ orbital decreases. As more protons occupy the $ \pi g_{9/2} $ orbital, the $ \nu g_{7/2} $ orbital is lowered because of the enhanced proton-neutron attraction resulting from the large wave-function overlap between these spin-orbit partners (see Ref. [9] and references therein).

In $ ^{{95}}\text{Tc} $ , breaking of the $ N=50 $ core was previously incorporated into shell-model calculations to describe high-spin states [6]. However, large discrepancies remain between theoretical and experimental level energies; these discrepancies were attributed to either the effective interactions or the limited model space used. Recent investigations indicate that neutron $ d_{5/2} \rightarrow g_{7/2} $ excitation is energetically more favorable than $ N=50 $ core breaking in the $ N=52 $ isotones [7−9]. Nevertheless, the $ d_{5/2} \rightarrow g_{7/2} $ excitation has not been included in calculations for $ ^{{95}}\text{Tc} $ , and the lack of experimental data in the corresponding energy region has further hindered understanding of the dominant excitation mechanisms.

The purpose of the present study is to probe these structural features in $ ^{{95}}\text{Tc} $ and to complete the systematics of $ d_{5/2} \rightarrow g_{7/2} $ excitations along the $ N=52 $ isotones, thereby contributing to a comprehensive understanding of nuclear structure in the $ A\sim 90 $ region. Prior to this work, low-spin states in $ ^{{95}}\text{Tc} $ were observed from electron capture (EC) and isomeric decay [18,19], as well as from transfer reaction experiments [20]. Previous high-spin work on⁹⁵Tc was reported by Ghugre et al. [6], who populated the nucleus through the (HI,α2n) side channel as a by-product of the (HI, xn) and (HI, pxn) reactions using the Early Implementation Gammasphere. Here, we report the experimental results for the high-spin level structure of $ ^{{95}}\text{Tc} $ obtained via in-beamγ-ray spectroscopy following a heavy-ion fusion-evaporation reaction.

High-spin states in⁹⁵Tc were populated via the⁸⁷Rb(¹²C, $ 4n $ )⁹⁵Tc fusion-evaporation reaction using a 62-MeV¹²C beam provided by the Sector Focusing Cyclotron at the Heavy Ion Research Facility in Lanzhou (HIRFL) [21]. The target consisted of an 18 μg/cm²C foil facing the beam, followed by an⁸⁷RbCl foil with a thickness of 4.2 mg/cm²and a natural Pb foil with a thickness of 8.7 mg/cm². The Pb foil served as the stopper for the reaction residues, and the C foil served as the covering layer for the hygroscopic⁸⁷RbCl foil. The emittedγrays were detected using a multi-detector array [22], which consisted of five Clover detectors of the EXOGAM type [23] grouped into a ring at $ 90^\circ $ and fourteen high-purity germanium (HPGe) detectors with a relative efficiency of 70% grouped into four rings at $ \pm52^\circ $ and $ \pm26^\circ $ relative to the beam axis. Specifically, four HPGe detectors were placed at each of $ 52^\circ $ and $ 26^\circ $ , and three were placed at each of $ 128^\circ $ and $ 154^\circ $ . All detectors were equipped with BGO anti-Compton shields. A total of 1.0 $ \times $ 10⁹γ-γ-γcoincidence events were recorded and sorted into a three-dimensional histogram (cube) for subsequent off-line analysis. In addition, $ 7\times10^{9} $ γ-γcoincidence events were recorded. In the experiment, the energy and efficiency calibrations were performed using⁶⁰Co,¹³³Ba, and¹⁵²Eu standard sources, and the typical energy resolution was about 2.0−2.5 keV at full width at half-maximum (FWHM) for the 1332.5-keVγray of⁶⁰Co.

To obtain angular distribution information for the emittedγrays,γ-ray angular distribution asymmetry ratios from oriented nuclei (ADO), $ R_{{\rm{ADO}}}(\gamma)=I_{\gamma}(\pm26^\circ)/ I_{\gamma}(90^\circ) $ , were extracted. Two asymmetric matrices were constructed using theγrays detected at all angles against those observed at $ \pm $ 26 $ ^\circ $ and 90 $ ^\circ $ , respectively. By setting gates on the axis with all detectors, theγ-ray intensities $ I_{\gamma} $ were extracted from the coincidence spectra regardless of the multipole character of the gating transition. Typical $ R_{{\rm{ADO}}}(\gamma) $ values were $ \approx 1.4 $ for stretched-quadrupole transitions (or unstretched dipole transitions) and $ \approx 0.8 $ for stretched-dipole transitions, as deduced from known transitions in nuclei produced in the present reaction.

The ADO ratio is mainly sensitive to the transition multipolarity,i.e., the dipole or quadrupole character. However, it does not provide direct information on the electric or magnetic nature of a transition. Therefore, stretchedM1/E2 mixed transitions and E1 transitions may not be unambiguously distinguished by ADO ratios alone. Consequently, parity assignments derived solely from ADO ratios, in the absence of complementary information such as linear-polarization measurements, must be regarded as tentative. A linear-polarization analysis using the present setup was not feasible because of limited statistics in the coincidence polarization matrices. Accordingly, when the ADO ratios alone are insufficient to determine the parity unambiguously, the parity assignments of the newly observed levels are given in parentheses throughout this work.

High-spin states in⁹⁵Tc were populated via the⁸⁷Rb(¹²C, $ 4n $ )⁹⁵Tc fusion-evaporation reaction using a 62-MeV¹²C beam provided by the Sector Focusing Cyclotron at the Heavy Ion Research Facility in Lanzhou (HIRFL) [21]. The target consisted of an 18 μg/cm²C foil facing the beam, followed by an⁸⁷RbCl foil with a thickness of 4.2 mg/cm²and a natural Pb foil with a thickness of 8.7 mg/cm². The Pb foil served as the stopper for the reaction residues, and the C foil served as the covering layer for the hygroscopic⁸⁷RbCl foil. The emittedγrays were detected using a multi-detector array [22], which consisted of five Clover detectors of the EXOGAM type [23] grouped into a ring at $ 90^\circ $ and fourteen high-purity germanium (HPGe) detectors with a relative efficiency of 70% grouped into four rings at $ \pm52^\circ $ and $ \pm26^\circ $ relative to the beam axis. Specifically, four HPGe detectors were placed at each of $ 52^\circ $ and $ 26^\circ $ , and three were placed at each of $ 128^\circ $ and $ 154^\circ $ . All detectors were equipped with BGO anti-Compton shields. A total of 1.0 $ \times $ 10⁹γ-γ-γcoincidence events were recorded and sorted into a three-dimensional histogram (cube) for subsequent off-line analysis. In addition, $ 7\times10^{9} $ γ-γcoincidence events were recorded. In the experiment, the energy and efficiency calibrations were performed using⁶⁰Co,¹³³Ba, and¹⁵²Eu standard sources, and the typical energy resolution was about 2.0−2.5 keV at full width at half-maximum (FWHM) for the 1332.5-keVγray of⁶⁰Co.

To obtain angular distribution information for the emittedγrays,γ-ray angular distribution asymmetry ratios from oriented nuclei (ADO), $ R_{{\rm{ADO}}}(\gamma)=I_{\gamma}(\pm26^\circ)/ I_{\gamma}(90^\circ) $ , were extracted. Two asymmetric matrices were constructed using theγrays detected at all angles against those observed at $ \pm $ 26 $ ^\circ $ and 90 $ ^\circ $ , respectively. By setting gates on the axis with all detectors, theγ-ray intensities $ I_{\gamma} $ were extracted from the coincidence spectra regardless of the multipole character of the gating transition. Typical $ R_{{\rm{ADO}}}(\gamma) $ values were $ \approx 1.4 $ for stretched-quadrupole transitions (or unstretched dipole transitions) and $ \approx 0.8 $ for stretched-dipole transitions, as deduced from known transitions in nuclei produced in the present reaction.

The ADO ratio is mainly sensitive to the transition multipolarity,i.e., the dipole or quadrupole character. However, it does not provide direct information on the electric or magnetic nature of a transition. Therefore, stretchedM1/E2 mixed transitions and E1 transitions may not be unambiguously distinguished by ADO ratios alone. Consequently, parity assignments derived solely from ADO ratios, in the absence of complementary information such as linear-polarization measurements, must be regarded as tentative. A linear-polarization analysis using the present setup was not feasible because of limited statistics in the coincidence polarization matrices. Accordingly, when the ADO ratios alone are insufficient to determine the parity unambiguously, the parity assignments of the newly observed levels are given in parentheses throughout this work.

Compared with the previous work of Ref. [6], 42 newγrays and 21 new levels have been incorporated into the level scheme of $ ^{{95}}\text{Tc} $ , as shown inFig. 1. The newly identified levels (transitions) and spin-parity assignments are indicated in red, and the revised spin-parity assignments are indicated in green. Representativeγ-ray coincidence spectra are presented inFig. 2. $ R_{{\rm{ADO}}} $ ratios of selected transitions in⁹⁵Tc are plotted as a function ofγ-ray energy inFig. 3. The measured spectroscopic data, includingγ-ray energies, relative intensities, $ R_{{\rm{ADO}}} $ ratios, multipolarities, and assigned level spin-parities, are summarized inTable 1. It should be noted that the relative intensities of the weakγrays listed inTable 1were extracted from the two-dimensional coincidence matrix, which provides higher statistics. In contrast, the coincidence spectra shown inFig. 2were generated from the three-dimensional coincidence cube with double gates to suppress contaminant transitions. Consequently, the apparent peak heights of some weak transitions inFig. 2may not directly reflect their relative intensities. These spectra are used mainly to establish coincidence relationships, whereas the relative intensities listed inTable 1were obtained from the two-dimensional coincidence matrix. Extensions and modifications of the level scheme are presented and discussed below.

Figure 1.(color online) Level scheme for⁹⁵Tc. Transitions newly observed in the present work are marked in red; spin-parity assignments that differ from those in Ref. [6] are marked in green. Transition energies are given in keV, and theγ-ray intensities are indicated by the arrow widths. Spin-parity values in parentheses are tentative.

Figure 2.(color online) Typical double-gated coincidence spectra obtained from the three-dimensional coincidence cube are shown. The spectra in panels (a) and (b) were obtained by summing spectra gated on the transition before the slash and on the transition(s) in parentheses. The newly observed transitions are marked in red.

Figure 3.(color online) The $ R_{ADO} $ values for selected transitions in⁹⁵Tc as a function ofγ-ray energy. Newly observed and previously reported transitions are indicated in red and black, respectively. The quoted uncertainties include contributions from background subtraction, fitting, and efficiency correction.

For the positive-parity states, the present level scheme is consistent with the work of Ref. [6] up to the 5600-keV level, whereas the 660-keVγray feeding the 2184-keV level reported in Ref. [6] cannot be confirmed. Thisγray can be traced back to the work of Sarantites [24], which reported a cascade of three strongγrays with energies of 663,634, and 592 keV feeding the $ 11/2^{+} $ state. Later, the 663-keV transition was found to decay from the 2213-keV state to the 1550-keV state, corresponding to a $ 17/2^{-}\rightarrow 15/2^{+} $ transition [25−27], as shown in the present level scheme. It seems unlikely that an intense 660-keV transition should be placed above the $ 19/2^{+} $ state with a sudden termination of theγ-ray flux [6].

Based on the measured $ R_{{\rm{ADO}}} $ value, we assigned E2 multipolarity to the 1682-keV transition. This assignment differs from the tentative M1 assignment in Ref. [6] but agrees with the angular-distribution results in Ref. [24], leading to the $ 33/2^{+} $ assignment for the 5600-keV level. Above this state, severalγrays with energies larger than 2 MeV are observed, as shown in the top right of the level scheme and inFig. 2(a).

The negative-parity states have been extended to an excitation energy of ~9.1 MeV based on the identification of new transitions, as shown inFig. 2(c). In addition, a sequence consisting of 656-, 582-, and 1134-keVγrays is firmly established above the 25/2 $ ^- $ state at 4127 keV through the observation of linking transitions connecting the negative- and positive-parity states. The $ R_{{\rm{ADO}}} $ value for the 306-keVγray depopulating the 25/2 $ ^- $ state is 1.35, consistent with an assignment of either a $ \Delta I =0 $ or $ \Delta I =2 $ transition, corresponding to a $ (25/2^-) $ or $ (29/2^{-}) $ assignment for the 4127-keV level. The latter can be ruled out because it would require anM2 multipolarity for the 611-keV transition, which could not compete with the presumed 306-keVE2 transition.

Compared with the previous work of Ref. [6], 42 newγrays and 21 new levels have been incorporated into the level scheme of $ ^{{95}}\text{Tc} $ , as shown inFig. 1. The newly identified levels (transitions) and spin-parity assignments are indicated in red, and the revised spin-parity assignments are indicated in green. Representativeγ-ray coincidence spectra are presented inFig. 2. $ R_{{\rm{ADO}}} $ ratios of selected transitions in⁹⁵Tc are plotted as a function ofγ-ray energy inFig. 3. The measured spectroscopic data, includingγ-ray energies, relative intensities, $ R_{{\rm{ADO}}} $ ratios, multipolarities, and assigned level spin-parities, are summarized inTable 1. It should be noted that the relative intensities of the weakγrays listed inTable 1were extracted from the two-dimensional coincidence matrix, which provides higher statistics. In contrast, the coincidence spectra shown inFig. 2were generated from the three-dimensional coincidence cube with double gates to suppress contaminant transitions. Consequently, the apparent peak heights of some weak transitions inFig. 2may not directly reflect their relative intensities. These spectra are used mainly to establish coincidence relationships, whereas the relative intensities listed inTable 1were obtained from the two-dimensional coincidence matrix. Extensions and modifications of the level scheme are presented and discussed below.

Figure 1.(color online) Level scheme for⁹⁵Tc. Transitions newly observed in the present work are marked in red; spin-parity assignments that differ from those in Ref. [6] are marked in green. Transition energies are given in keV, and theγ-ray intensities are indicated by the arrow widths. Spin-parity values in parentheses are tentative.

Figure 2.(color online) Typical double-gated coincidence spectra obtained from the three-dimensional coincidence cube are shown. The spectra in panels (a) and (b) were obtained by summing spectra gated on the transition before the slash and on the transition(s) in parentheses. The newly observed transitions are marked in red.

Figure 3.(color online) The $ R_{ADO} $ values for selected transitions in⁹⁵Tc as a function ofγ-ray energy. Newly observed and previously reported transitions are indicated in red and black, respectively. The quoted uncertainties include contributions from background subtraction, fitting, and efficiency correction.

For the positive-parity states, the present level scheme is consistent with the work of Ref. [6] up to the 5600-keV level, whereas the 660-keVγray feeding the 2184-keV level reported in Ref. [6] cannot be confirmed. Thisγray can be traced back to the work of Sarantites [24], which reported a cascade of three strongγrays with energies of 663,634, and 592 keV feeding the $ 11/2^{+} $ state. Later, the 663-keV transition was found to decay from the 2213-keV state to the 1550-keV state, corresponding to a $ 17/2^{-}\rightarrow 15/2^{+} $ transition [25−27], as shown in the present level scheme. It seems unlikely that an intense 660-keV transition should be placed above the $ 19/2^{+} $ state with a sudden termination of theγ-ray flux [6].

Based on the measured $ R_{{\rm{ADO}}} $ value, we assigned E2 multipolarity to the 1682-keV transition. This assignment differs from the tentative M1 assignment in Ref. [6] but agrees with the angular-distribution results in Ref. [24], leading to the $ 33/2^{+} $ assignment for the 5600-keV level. Above this state, severalγrays with energies larger than 2 MeV are observed, as shown in the top right of the level scheme and inFig. 2(a).

The negative-parity states have been extended to an excitation energy of ~9.1 MeV based on the identification of new transitions, as shown inFig. 2(c). In addition, a sequence consisting of 656-, 582-, and 1134-keVγrays is firmly established above the 25/2 $ ^- $ state at 4127 keV through the observation of linking transitions connecting the negative- and positive-parity states. The $ R_{{\rm{ADO}}} $ value for the 306-keVγray depopulating the 25/2 $ ^- $ state is 1.35, consistent with an assignment of either a $ \Delta I =0 $ or $ \Delta I =2 $ transition, corresponding to a $ (25/2^-) $ or $ (29/2^{-}) $ assignment for the 4127-keV level. The latter can be ruled out because it would require anM2 multipolarity for the 611-keV transition, which could not compete with the presumed 306-keVE2 transition.

Spherical shell-model calculations were performed to interpret the level structures of the $ N=52 $ isotones from $ ^{{90}}\text{Sr} $ to $ ^{{97}}\text{Rh} $ [4−8,10,16,28]. For $ ^{{95}}\text{Tc} $ , the low-lying states up to spin $ 29/2 $ were reasonably described using a model space of $ \pi (p_{1/2}, g_{9/2}) $ and $ \nu (d_{5/2}, s_{1/2}) $ with an inert $ ^{{88}}\text{Sr} $ core [6]. However, significant discrepancies between predictions and observations were found for the high-spin states because of the limited model space. These discrepancies remained unresolved, even when $ N = 50 $ core breaking was included in the calculation [6].

Recent studies of the neighboring nucleus $ ^{{93}}\text{Nb} $ indicated that breaking of the $ N=50 $ core occurs only for states above the $ 41/2^{-} $ state at an excitation energy of ~9.1 MeV. In contrast, neutron $ d_{5/2} \rightarrow g_{7/2} $ excitations were found to occur at relatively low excitation energies for both positive- and negative-parity states [8]. Similar systematics were observed in other $ N=52 $ isotones, such as $ ^{{92}}\text{Zr} $ [9] and $ ^{{94}}\text{Mo} $ [7]. Indeed, the energy required for the neutron $ d_{5/2} \rightarrow g_{7/2} $ excitation was identified to be around $ 1.6 $ MeV [7,9], which is notably close to the energy of the 1682-keV transition feeding the $ 29/2^+ $ state in $ ^{{95}}\text{Tc} $ . These systematic features emphasize the need to include such excitations explicitly in the calculations.

In the present work, new transitions have been identified, particularly above the $ 29/2^{\pm} $ states. To interpret these states, shell-model calculations were performed using the kshell code [29] within an enlarged model space that includes both the neutron $ d_{5/2} \rightarrow g_{7/2} $ excitation and neutron $ N=50 $ core breaking. The model space includes four proton orbitals $ (f_{5/2},p_{3/2},p_{1/2},g_{9/2}) $ and seven neutron orbitals $ (f_{5/2},p_{3/2},p_{1/2},g_{9/2}, d_{5/2}, g_{7/2},s_{1/2}) $ . The Hamiltonian within the $ f_5pg_{9} $ shell employs the JUN45 interaction [30], whereas the remaining matrix elements are derived from the V $ {\rm{}}_{MU} $ interaction. Owing to computational limitations, at most one neutron is allowed to be excited from the $ f_5pg_{9} $ shell to the $ g_{7/2} $ , $ d_{5/2} $ , or $ s_{1/2} $ orbitals [31]. The largest M-scheme dimension under this $ 1p-1h $ truncation is approximately $ 6.7\times10^{7} $ .

Before comparing the experimental level scheme with the shell-model calculations, we comment on the robustness of the spin-parity assignments. The ADO analysis described in Section III provides reliable discrimination among stretched dipole ( $ \Delta J = 1 $ ), stretched quadrupole ( $ \Delta J = 2 $ ), and $ \Delta J = 0 $ transitions, but it cannot distinguishE1 fromM1/E2 character on a transition-by-transition basis. Consequently, the parities of several newly proposed levels cannot be firmly established from the present data alone. These include the parities of the $ (25/2^-) $ level at 4127 keV, the $ (31/2^-) $ level at 5729 keV and the higher-lying level at 6570 keV that feeds it, the $ (35/2^-) $ level at 7803 keV and the levels at 8554 and 9078 keV, the $ (35/2^+) $ level at 7906 keV, and the $ (39/2^-) $ level at 8361 keV. These assignments should therefore be regarded as tentative.

A comparison between the experimental excitation energies and the shell-model predictions for the levels in $ ^{{95}}\text{Tc} $ is presented inFig. 4. For a given spin and parity, the shell-model calculations often predict several states close in energy. Throughout this work, the experimental levels are matched to the calculated states on the basis of the ordering of excitation energies and the yrast-population criterion. When only one experimental level is known for a given $ J^\pi $ , it is associated with the lowest calculated state. When two or more experimental levels are observed, they are matched to the calculated states in increasing order of excitation energy. The calculated transition probabilities for the high-lying states are subject to larger uncertainties because of the model-space truncation; therefore, the correspondence is established primarily on the basis of excitation energies and decay patterns rather thanB(M1) orB(E2) values. The calculated levels show reasonable agreement with the experimental data, particularly for the low-lying states up to ~4 MeV. Above this energy, the discrepancies increase, especially for the negative-parity states. The dominant wave functions and seniorities of the positive- and negative-parity states are listed inTables 2and3, respectively. Here, the M-scheme many-body wave functions are expanded in an orbit-wise seniority basis and classified by proton seniority $ \nu_p $ and neutron seniority $ \nu_n $ , obtained by summing the seniorities over the proton and neutron orbitals, respectively.

Figure 4.(color online) Comparison of experimental levels in⁹⁵Tc with shell-model predictions. As inFig. 1, newly observed levels are indicated in red, and levels with revised spin-parity assignments are shown in green. Tentative spin-parity assignments are shown in parentheses.

For positive-parity states, the $ 9/2^+ $ ground state is dominated by a single proton in the $ g_{9/2} $ orbital with seniority $ \nu = 1 $ . This state is followed by a group of seniority-three states based on the configuration of one $ g_{9/2} $ proton coupled to a broken neutron pair in the $ d_{5/2} $ orbital,i.e., $ \nu d_{5/2}^2 $ , up to the $ 17/2^+ $ state. In particular, the 882-keV energy of the $ 13/2^{+} $ state in⁹⁵Tc is very close to those of the $ 2^{+} $ states in the even-even $ N=52 $ isotones,i.e., 831, 934, 871, and 833 keV in⁹⁰Sr [12−14],⁹²Zr [9],⁹⁴Mo [7], and⁹⁶Ru [5], respectively. The predominant configuration of these $ 2^{+} $ states is $ \nu d_{5/2}^2 $ . The $ 19/2^+ $ and $ 21/2^+ $ states are predicted to involve mainly the $ \nu (d_{5/2}g_{7/2}) $ component. This indicates that the neutron $ d_{5/2} \rightarrow g_{7/2} $ excitation begins at an excitation energy of ~2.2 MeV. Above the three-particle fully aligned $ 21/2^{+} $ state, an additional nucleon pair must be broken to generate further excitations. The higher-spin states therefore have seniority-5 configurations. Shell-model calculations predict that the breaking of a $ \pi g_{9/2} $ pair is responsible for the states up to the $ 33/2^+ $ state. Above this state, proton excitations from the $ f_{5/2} $ or $ p_{3/2} $ orbitals across the $ Z=38 $ shell to the $ g_{9/2} $ orbital become important. Among the transitions depopulating the levels around 7800−7900 keV, the 2306-keVγray is the strongest, suggesting that the 7906-keV level depopulated by this transition is more likely to be the yrast $ (35/2^+) $ state, consistent with the yrast-population criterion discussed above.

It should be noted that although the ADO ratios of the 667.3- and 668.5-keV transitions are close to the values expected forE2 radiation, both transitions connect states with $ \Delta I $ =1 and are assigned as mixedM1/E2 transitions. According to the shell-model calculations, the 668.5-keV transition involves a change in the dominant neutron occupation from $ \nu(g_{7/2}d_{5/2}) $ to $ \nu(d_{5/2}^2) $ . The corresponding $ g_{7/2}\rightarrow d_{5/2} $ neutron transition has $ \Delta l=2 $ , making theM1 componentl-forbidden and strongly hindered. The relativeE2 contribution can therefore be substantial, resulting in anE2-like ADO ratio. In contrast, the states connected by the 667.3-keV transition have similar proton and neutron orbital occupancies but may differ in the angular-momentum coupling of the proton configuration. The transition could thus be regarded as occurring between different proton-coupling multiplets, for which a sizableE2 admixture is consistent with the observed ADO ratio.

As shown inTable 3, the dominant proton contribution to nearly all negative-parity states includes a particle occupying the $ p_{1/2} $ orbital. The lowest $ 1/2^- $ state has the pure single-particle configuration $ \pi p_{1/2} $ . The $ 5/2^- $ , $ 9/2^- $ , and $ 17/2^- $ states mainly arise from the coupling of $ \pi p_{1/2} $ to a broken proton pair in the $ g_{9/2} $ orbital, whereas the $ 13/2^- $ state arises from the coupling of $ \pi p_{1/2} $ with two neutrons in the $ \nu (d_{5/2} g_{7/2}) $ configuration. This indicates that the neutron $ d_{5/2} \rightarrow g_{7/2} $ excitation occurs at ~1.7 MeV, lower than that in positive-parity states (~2.2 MeV). For the higher-lying states, the dominant configuration is $ \pi (p_{1/2}g_{9/2})^5\otimes \nu (d_{5/2}/g_{7/2})^2 $ with a seniority of 7. The maximum angular momentum of this configuration is $ 37/2^{-} $ . Therefore, excitation of a proton from the $ \pi p_{3/2} $ orbital and subsequently from the $ \pi f_{5/2} $ orbital into the $ \pi g_{9/2} $ orbital is necessary to form the even higher-spin states with $ J=39/2 $ and $ J=41/2 $ , respectively. In addition, shell-model calculations predict several $ 43/2 $ states dominated by the $ N=50 $ core excitation, but they are not observed experimentally.

Spherical shell-model calculations were performed to interpret the level structures of the $ N=52 $ isotones from $ ^{{90}}\text{Sr} $ to $ ^{{97}}\text{Rh} $ [4−8,10,16,28]. For $ ^{{95}}\text{Tc} $ , the low-lying states up to spin $ 29/2 $ were reasonably described using a model space of $ \pi (p_{1/2}, g_{9/2}) $ and $ \nu (d_{5/2}, s_{1/2}) $ with an inert $ ^{{88}}\text{Sr} $ core [6]. However, significant discrepancies between predictions and observations were found for the high-spin states because of the limited model space. These discrepancies remained unresolved, even when $ N = 50 $ core breaking was included in the calculation [6].

Recent studies of the neighboring nucleus $ ^{{93}}\text{Nb} $ indicated that breaking of the $ N=50 $ core occurs only for states above the $ 41/2^{-} $ state at an excitation energy of ~9.1 MeV. In contrast, neutron $ d_{5/2} \rightarrow g_{7/2} $ excitations were found to occur at relatively low excitation energies for both positive- and negative-parity states [8]. Similar systematics were observed in other $ N=52 $ isotones, such as $ ^{{92}}\text{Zr} $ [9] and $ ^{{94}}\text{Mo} $ [7]. Indeed, the energy required for the neutron $ d_{5/2} \rightarrow g_{7/2} $ excitation was identified to be around $ 1.6 $ MeV [7,9], which is notably close to the energy of the 1682-keV transition feeding the $ 29/2^+ $ state in $ ^{{95}}\text{Tc} $ . These systematic features emphasize the need to include such excitations explicitly in the calculations.

In the present work, new transitions have been identified, particularly above the $ 29/2^{\pm} $ states. To interpret these states, shell-model calculations were performed using the kshell code [29] within an enlarged model space that includes both the neutron $ d_{5/2} \rightarrow g_{7/2} $ excitation and neutron $ N=50 $ core breaking. The model space includes four proton orbitals $ (f_{5/2},p_{3/2},p_{1/2},g_{9/2}) $ and seven neutron orbitals $ (f_{5/2},p_{3/2},p_{1/2},g_{9/2}, d_{5/2}, g_{7/2},s_{1/2}) $ . The Hamiltonian within the $ f_5pg_{9} $ shell employs the JUN45 interaction [30], whereas the remaining matrix elements are derived from the V $ {\rm{}}_{MU} $ interaction. Owing to computational limitations, at most one neutron is allowed to be excited from the $ f_5pg_{9} $ shell to the $ g_{7/2} $ , $ d_{5/2} $ , or $ s_{1/2} $ orbitals [31]. The largest M-scheme dimension under this $ 1p-1h $ truncation is approximately $ 6.7\times10^{7} $ .

Before comparing the experimental level scheme with the shell-model calculations, we comment on the robustness of the spin-parity assignments. The ADO analysis described in Section III provides reliable discrimination among stretched dipole ( $ \Delta J = 1 $ ), stretched quadrupole ( $ \Delta J = 2 $ ), and $ \Delta J = 0 $ transitions, but it cannot distinguishE1 fromM1/E2 character on a transition-by-transition basis. Consequently, the parities of several newly proposed levels cannot be firmly established from the present data alone. These include the parities of the $ (25/2^-) $ level at 4127 keV, the $ (31/2^-) $ level at 5729 keV and the higher-lying level at 6570 keV that feeds it, the $ (35/2^-) $ level at 7803 keV and the levels at 8554 and 9078 keV, the $ (35/2^+) $ level at 7906 keV, and the $ (39/2^-) $ level at 8361 keV. These assignments should therefore be regarded as tentative.

A comparison between the experimental excitation energies and the shell-model predictions for the levels in $ ^{{95}}\text{Tc} $ is presented inFig. 4. For a given spin and parity, the shell-model calculations often predict several states close in energy. Throughout this work, the experimental levels are matched to the calculated states on the basis of the ordering of excitation energies and the yrast-population criterion. When only one experimental level is known for a given $ J^\pi $ , it is associated with the lowest calculated state. When two or more experimental levels are observed, they are matched to the calculated states in increasing order of excitation energy. The calculated transition probabilities for the high-lying states are subject to larger uncertainties because of the model-space truncation; therefore, the correspondence is established primarily on the basis of excitation energies and decay patterns rather thanB(M1) orB(E2) values. The calculated levels show reasonable agreement with the experimental data, particularly for the low-lying states up to ~4 MeV. Above this energy, the discrepancies increase, especially for the negative-parity states. The dominant wave functions and seniorities of the positive- and negative-parity states are listed inTables 2and3, respectively. Here, the M-scheme many-body wave functions are expanded in an orbit-wise seniority basis and classified by proton seniority $ \nu_p $ and neutron seniority $ \nu_n $ , obtained by summing the seniorities over the proton and neutron orbitals, respectively.

Figure 4.(color online) Comparison of experimental levels in⁹⁵Tc with shell-model predictions. As inFig. 1, newly observed levels are indicated in red, and levels with revised spin-parity assignments are shown in green. Tentative spin-parity assignments are shown in parentheses.

For positive-parity states, the $ 9/2^+ $ ground state is dominated by a single proton in the $ g_{9/2} $ orbital with seniority $ \nu = 1 $ . This state is followed by a group of seniority-three states based on the configuration of one $ g_{9/2} $ proton coupled to a broken neutron pair in the $ d_{5/2} $ orbital,i.e., $ \nu d_{5/2}^2 $ , up to the $ 17/2^+ $ state. In particular, the 882-keV energy of the $ 13/2^{+} $ state in⁹⁵Tc is very close to those of the $ 2^{+} $ states in the even-even $ N=52 $ isotones,i.e., 831, 934, 871, and 833 keV in⁹⁰Sr [12−14],⁹²Zr [9],⁹⁴Mo [7], and⁹⁶Ru [5], respectively. The predominant configuration of these $ 2^{+} $ states is $ \nu d_{5/2}^2 $ . The $ 19/2^+ $ and $ 21/2^+ $ states are predicted to involve mainly the $ \nu (d_{5/2}g_{7/2}) $ component. This indicates that the neutron $ d_{5/2} \rightarrow g_{7/2} $ excitation begins at an excitation energy of ~2.2 MeV. Above the three-particle fully aligned $ 21/2^{+} $ state, an additional nucleon pair must be broken to generate further excitations. The higher-spin states therefore have seniority-5 configurations. Shell-model calculations predict that the breaking of a $ \pi g_{9/2} $ pair is responsible for the states up to the $ 33/2^+ $ state. Above this state, proton excitations from the $ f_{5/2} $ or $ p_{3/2} $ orbitals across the $ Z=38 $ shell to the $ g_{9/2} $ orbital become important. Among the transitions depopulating the levels around 7800−7900 keV, the 2306-keVγray is the strongest, suggesting that the 7906-keV level depopulated by this transition is more likely to be the yrast $ (35/2^+) $ state, consistent with the yrast-population criterion discussed above.

It should be noted that although the ADO ratios of the 667.3- and 668.5-keV transitions are close to the values expected forE2 radiation, both transitions connect states with $ \Delta I $ =1 and are assigned as mixedM1/E2 transitions. According to the shell-model calculations, the 668.5-keV transition involves a change in the dominant neutron occupation from $ \nu(g_{7/2}d_{5/2}) $ to $ \nu(d_{5/2}^2) $ . The corresponding $ g_{7/2}\rightarrow d_{5/2} $ neutron transition has $ \Delta l=2 $ , making theM1 componentl-forbidden and strongly hindered. The relativeE2 contribution can therefore be substantial, resulting in anE2-like ADO ratio. In contrast, the states connected by the 667.3-keV transition have similar proton and neutron orbital occupancies but may differ in the angular-momentum coupling of the proton configuration. The transition could thus be regarded as occurring between different proton-coupling multiplets, for which a sizableE2 admixture is consistent with the observed ADO ratio.

As shown inTable 3, the dominant proton contribution to nearly all negative-parity states includes a particle occupying the $ p_{1/2} $ orbital. The lowest $ 1/2^- $ state has the pure single-particle configuration $ \pi p_{1/2} $ . The $ 5/2^- $ , $ 9/2^- $ , and $ 17/2^- $ states mainly arise from the coupling of $ \pi p_{1/2} $ to a broken proton pair in the $ g_{9/2} $ orbital, whereas the $ 13/2^- $ state arises from the coupling of $ \pi p_{1/2} $ with two neutrons in the $ \nu (d_{5/2} g_{7/2}) $ configuration. This indicates that the neutron $ d_{5/2} \rightarrow g_{7/2} $ excitation occurs at ~1.7 MeV, lower than that in positive-parity states (~2.2 MeV). For the higher-lying states, the dominant configuration is $ \pi (p_{1/2}g_{9/2})^5\otimes \nu (d_{5/2}/g_{7/2})^2 $ with a seniority of 7. The maximum angular momentum of this configuration is $ 37/2^{-} $ . Therefore, excitation of a proton from the $ \pi p_{3/2} $ orbital and subsequently from the $ \pi f_{5/2} $ orbital into the $ \pi g_{9/2} $ orbital is necessary to form the even higher-spin states with $ J=39/2 $ and $ J=41/2 $ , respectively. In addition, shell-model calculations predict several $ 43/2 $ states dominated by the $ N=50 $ core excitation, but they are not observed experimentally.

As shown inTable 2, the $ 29/2^+ $ and $ 33/2^+ $ states, while having identical proton configurations, are characterized by relatively pure neutron components: predominantly $ \nu d_{5/2}^2 $ for the former and $ \nu (d_{5/2}g_{7/2}) $ for the latter. The 1682-keV transition between them therefore provides an excellent example of the $ d_{5/2} \rightarrow g_{7/2} $ excitation.

In the framework of the spin-isospin-dependent central force [32−34], the enhanced $ \pi g_{9/2}-\nu g_{7/2} $ monopole interaction lowers the energy of the $ \nu g_{7/2} $ orbital, leading to a $ \nu (d_{5/2} \rightarrow g_{7/2}) $ excitation of ~1.0 MeV in $ N=52 $ isotones with $ 38[9,35]. Specifically, in⁹²Zr and⁹³Nb, the yrast $ (12^{+})\rightarrow (14^{+}) $ and $ 29/2^{(+)}\rightarrow33/2^{(+)} $ excitations are attributed to the $ \nu (d_{5/2} \rightarrow g_{7/2}) $ excitations, with corresponding transition energies of 1098 [9] and 1040 keV [35], as shown inFig. 5. However, the energy required for the $ 29/2^{+}\rightarrow33/2^{+} $ excitation in⁹⁵Tc is 1682 keV, substantially larger than expected. This value closely matches that of the adjacent even-even core nucleus⁹⁴Mo (1609 keV,Fig. 5). These four nuclei can therefore be classified into two groups:⁹⁵Tc and⁹⁴Mo, which exhibit unexpectedly high excitation energies, and $ ^{{92}}\text{Zr} $ and $ ^{{93}}\text{Nb} $ , which belong to the other category. The increase in excitation energy may be accounted for by configuration mixing, as discussed below.

Figure 5.Comparison of the excitation energies of positive-parity states in $ N=52 $ isotones. All states in⁹⁴Mo (⁹⁵Tc) lie systematically lower in energy than these corresponding states in⁹²Zr (⁹³Nb). The only exceptions are the $ 4^{+} $ and $ 17/2^{+} $ states, which may be attributed to their pure, fully aligned configurations, $ \nu (d_{5/2}^2)_{4^{+}} $ and $ \pi g_{9/2}\otimes \nu (d_{5/2}^2)_{4^{+}} $ , respectively. The data for⁹⁵Tc are from this work, whereas those for the other isotopes are from the following Refs.:⁹²Zr [9],⁹³Nb [8], and⁹⁴Mo [7].

We begin with the even-even nucleus⁹²Zr, which can be readily described as two protons and two neutrons outside the⁸⁸Sr core. The aforementioned $ 12^{+} $ level is the fully aligned four-particle state based on the pure configuration $ \pi (g_{9/2})^2_{8^+} \otimes \nu (d_{5/2})^2_{4^+} $ . Similarly, the $ 29/2^{+} $ state in⁹³Nb is expected to arise from the pure configuration involving an additional $ \pi g_{9/2} $ valence proton. In⁹⁴Mo, four protons are available outside the⁸⁸Sr core. Two $ 12^{+} $ states can be generated by coupling $ \pi (g_{9/2}^2)_{8^+} $ or $ \pi (g_{9/2}^4)_{8^+} $ to $ \nu (d_{5/2}^2)_{4^+} $ , respectively. Configuration mixing produces repulsion between the two intrinsic states, lowering the lower level and raising the higher level in energy. Furthermore, when only two $ g_{9/2} $ protons are aligned, the pairing interaction (pairing scattering) could occur between $ \pi (g_{9/2}^2)_{0^{+}} $ and $ \pi (p_{1/2}^2)_{0^{+}} $ [36], leading to enhanced level repulsion. As shown inFig. 5, the level repulsion lowers the $ 12^{+} $ and $ 29/2^{+} $ states, as well as all the states below them, relative to the corresponding states in⁹²Zr and⁹³Nb, respectively.

It should be noted that the pairing-scattering mechanism qualitatively explains the systematic lowering of many states in⁹⁴Mo and⁹⁵Tc compared with⁹²Zr and⁹³Nb. However, this simple picture encounters difficulties when examined in detail. The 29/2 $ ^+ $ state in⁹⁵Tc has a remarkably pure dominant configuration (71%, seeTable 2), suggesting a relatively pure state that should not be strongly affected by configuration mixing. Nevertheless, the $ 29/2^+\rightarrow33/2^+ $ energy gap is exceptionally large (1682 keV), indicating that this state has undergone a substantial downward shift. This inconsistency, together with the observation that the 4 $ ^+ $ and 17/2 $ ^+ $ states are actually higher in⁹⁴Mo and⁹⁵Tc, indicates that the simple two-state repulsion picture is incomplete.

As shown inTable 2, the $ 29/2^+ $ and $ 33/2^+ $ states, while having identical proton configurations, are characterized by relatively pure neutron components: predominantly $ \nu d_{5/2}^2 $ for the former and $ \nu (d_{5/2}g_{7/2}) $ for the latter. The 1682-keV transition between them therefore provides an excellent example of the $ d_{5/2} \rightarrow g_{7/2} $ excitation.

In the framework of the spin-isospin-dependent central force [32−34], the enhanced $ \pi g_{9/2}-\nu g_{7/2} $ monopole interaction lowers the energy of the $ \nu g_{7/2} $ orbital, leading to a $ \nu (d_{5/2} \rightarrow g_{7/2}) $ excitation of ~1.0 MeV in $ N=52 $ isotones with $ 38[9,35]. Specifically, in⁹²Zr and⁹³Nb, the yrast $ (12^{+})\rightarrow (14^{+}) $ and $ 29/2^{(+)}\rightarrow33/2^{(+)} $ excitations are attributed to the $ \nu (d_{5/2} \rightarrow g_{7/2}) $ excitations, with corresponding transition energies of 1098 [9] and 1040 keV [35], as shown inFig. 5. However, the energy required for the $ 29/2^{+}\rightarrow33/2^{+} $ excitation in⁹⁵Tc is 1682 keV, substantially larger than expected. This value closely matches that of the adjacent even-even core nucleus⁹⁴Mo (1609 keV,Fig. 5). These four nuclei can therefore be classified into two groups:⁹⁵Tc and⁹⁴Mo, which exhibit unexpectedly high excitation energies, and $ ^{{92}}\text{Zr} $ and $ ^{{93}}\text{Nb} $ , which belong to the other category. The increase in excitation energy may be accounted for by configuration mixing, as discussed below.

Figure 5.Comparison of the excitation energies of positive-parity states in $ N=52 $ isotones. All states in⁹⁴Mo (⁹⁵Tc) lie systematically lower in energy than these corresponding states in⁹²Zr (⁹³Nb). The only exceptions are the $ 4^{+} $ and $ 17/2^{+} $ states, which may be attributed to their pure, fully aligned configurations, $ \nu (d_{5/2}^2)_{4^{+}} $ and $ \pi g_{9/2}\otimes \nu (d_{5/2}^2)_{4^{+}} $ , respectively. The data for⁹⁵Tc are from this work, whereas those for the other isotopes are from the following Refs.:⁹²Zr [9],⁹³Nb [8], and⁹⁴Mo [7].

We begin with the even-even nucleus⁹²Zr, which can be readily described as two protons and two neutrons outside the⁸⁸Sr core. The aforementioned $ 12^{+} $ level is the fully aligned four-particle state based on the pure configuration $ \pi (g_{9/2})^2_{8^+} \otimes \nu (d_{5/2})^2_{4^+} $ . Similarly, the $ 29/2^{+} $ state in⁹³Nb is expected to arise from the pure configuration involving an additional $ \pi g_{9/2} $ valence proton. In⁹⁴Mo, four protons are available outside the⁸⁸Sr core. Two $ 12^{+} $ states can be generated by coupling $ \pi (g_{9/2}^2)_{8^+} $ or $ \pi (g_{9/2}^4)_{8^+} $ to $ \nu (d_{5/2}^2)_{4^+} $ , respectively. Configuration mixing produces repulsion between the two intrinsic states, lowering the lower level and raising the higher level in energy. Furthermore, when only two $ g_{9/2} $ protons are aligned, the pairing interaction (pairing scattering) could occur between $ \pi (g_{9/2}^2)_{0^{+}} $ and $ \pi (p_{1/2}^2)_{0^{+}} $ [36], leading to enhanced level repulsion. As shown inFig. 5, the level repulsion lowers the $ 12^{+} $ and $ 29/2^{+} $ states, as well as all the states below them, relative to the corresponding states in⁹²Zr and⁹³Nb, respectively.

It should be noted that the pairing-scattering mechanism qualitatively explains the systematic lowering of many states in⁹⁴Mo and⁹⁵Tc compared with⁹²Zr and⁹³Nb. However, this simple picture encounters difficulties when examined in detail. The 29/2 $ ^+ $ state in⁹⁵Tc has a remarkably pure dominant configuration (71%, seeTable 2), suggesting a relatively pure state that should not be strongly affected by configuration mixing. Nevertheless, the $ 29/2^+\rightarrow33/2^+ $ energy gap is exceptionally large (1682 keV), indicating that this state has undergone a substantial downward shift. This inconsistency, together with the observation that the 4 $ ^+ $ and 17/2 $ ^+ $ states are actually higher in⁹⁴Mo and⁹⁵Tc, indicates that the simple two-state repulsion picture is incomplete.

The high-spin levels in⁹⁵Tc have been studied using in-beamγ-ray spectroscopy via the⁸⁷Rb(¹²C, $ 4n $ )⁹⁵Tc fusion-evaporation reaction. The level scheme has been extended by 42γtransitions, reaching an excitation energy of ~9 MeV. Large-scale shell-model calculations have been performed and reproduce the experimental levels with good accuracy, providing a consistent interpretation of the observed level structure. The low-lying states in⁹⁵Tc are described by a proton in the $ (p_{1/2}, g_{9/2}) $ orbitals coupled to $ d_{5/2} $ neutrons, with an inert⁸⁸Sr core. With increasing excitation energy, $ d_{5/2} \rightarrow g_{7/2} $ neutron excitations are involved, beginning at excitation energies of 2184 keV and 1702 keV for positive- and negative-parity states, respectively. For the higher-spin states above the maximum angular momentum available from these active orbitals, breaking of the $ Z=38 $ subshell occurs. Proton excitations ( $ \pi f_{5/2} / p_{3/2}\rightarrow g_{9/2} $ ) coupled with neutron $ d_{5/2} \rightarrow g_{7/2} $ excitations result inγtransitions with energies greater than 2 MeV. Future experiments with higher statistics may help identify possible 2-MeV transitions associated with $ N=50 $ core breaking, which are expected to be off-yrast. In the present work, no clear evidence for $ N = 50 $ core breaking is observed up to excitation energies of 9 MeV.

The high-spin levels in⁹⁵Tc have been studied using in-beamγ-ray spectroscopy via the⁸⁷Rb(¹²C, $ 4n $ )⁹⁵Tc fusion-evaporation reaction. The level scheme has been extended by 42γtransitions, reaching an excitation energy of ~9 MeV. Large-scale shell-model calculations have been performed and reproduce the experimental levels with good accuracy, providing a consistent interpretation of the observed level structure. The low-lying states in⁹⁵Tc are described by a proton in the $ (p_{1/2}, g_{9/2}) $ orbitals coupled to $ d_{5/2} $ neutrons, with an inert⁸⁸Sr core. With increasing excitation energy, $ d_{5/2} \rightarrow g_{7/2} $ neutron excitations are involved, beginning at excitation energies of 2184 keV and 1702 keV for positive- and negative-parity states, respectively. For the higher-spin states above the maximum angular momentum available from these active orbitals, breaking of the $ Z=38 $ subshell occurs. Proton excitations ( $ \pi f_{5/2} / p_{3/2}\rightarrow g_{9/2} $ ) coupled with neutron $ d_{5/2} \rightarrow g_{7/2} $ excitations result inγtransitions with energies greater than 2 MeV. Future experiments with higher statistics may help identify possible 2-MeV transitions associated with $ N=50 $ core breaking, which are expected to be off-yrast. In the present work, no clear evidence for $ N = 50 $ core breaking is observed up to excitation energies of 9 MeV.