Quantum Behavior of Spin-Orbit Inelastic Scattering of C-Atoms by D2 at Low Energy

Fine-structure populations and collision–induced energy transfer in atoms are of interest for many fields, from combustion to astrophysics. In particular, neutral carbon atoms are known to play a role in interstellar media, either as probes of physical conditions (ground state 3Pj spin-orbit populations), or as cooling agent (collisional excitation followed by radiative decay). This work aims at investigating the spin-orbit excitation of atomic carbon in its ground electronic state due to collisions with molecular deuterium, an isotopic variant of H2, the most abundant molecule in the interstellar medium. Spin-orbit excitations of C(3Pj) by H2 or D2 are governed by non-adiabatic and spin-orbit couplings, which make the theoretical treatment challenging, since the Born-Oppenheimer approximation no longer holds. Inelastic collisional cross-sections were determined for the C(3P0) + D2 → C(3Pj) + D2 (with j = 1 and 2) excitation process. Experimental data were acquired in a crossed beam experiment at low collision energies, down to the excitation thresholds (at 16.42 and 43.41 cm−1, respectively). C-atoms were produced mainly in their ground spin-orbit state, 3P0, by dissociation of CO in a dielectric discharge through an Even-Lavie pulsed valve. The C-atom beam was crossed with a D2 beam from a second valve. The state-to-state cross-sections were derived from the C(3Pj) (j = 1 or 2) signal measured as a function of the beam crossing angle, i.e., as a function of the collision energy. The results show different quantum behaviors for excitation to C(3P1) or C(3P2) when C(3P0) collides with ortho-D2 or normal-D2. These experimental results are analyzed and discussed in the light of highly accurate quantum calculations. A good agreement between experimental and theoretical results is found. The present data are compared with those obtained for the C-He and C-H2 collisional systems to get new insights into the dynamics of collision induced spin-orbit excitation/relaxation of atomic carbon.


INTRODUCTION
Processes controlling internal state population distributions of atomic or molecular species are of interest in many fields. This is especially the case for astrophysics. In particular, information concerning the physical conditions prevailing in interstellar media can only be retrieved from spectra yielding the internal states relative populations of the observed species, which result from the equilibrium between collisional and radiative processes. For that purpose, neutral carbon atoms are of particular interest, since they are known to play a role in interstellar media, either as probes of physical conditions (ground state 3 P j spinorbit populations), or as a cooling agent (collisional excitation followed by a radiative decay). Indeed, C atoms are very abundant in many interstellar regions ranging from dense molecular clouds to planetary nebulae (Zmuidzinas et al., 1988;Bensby and Feltzing, 2006;Herbst and Yates, 2013). Hence, modeling the fine-structure population of C atoms is of major interest for astrochemical models. Such models rely on both collisional and radiative data. Collisional cross-sections and rate coefficients implying the C atoms and the dominant collisional partners in the interstellar medium (H 2 , He, H) have then to be determined at low temperatures. However, when molecular collisions (reactive or inelastic) occur at low energy/temperature, in the near cold regime (1-50 K), resonances are predicted by theory for many systems. Such resonances have been clearly observed in the collision energy dependent integral crosssections (ICS) for spin-orbit excitation of C( 3 P 0 ) by collisions with He  and H 2 . These processes are governed by non-adiabatic and spin-orbit couplings, which makes the theoretical treatment challenging since the Born-Oppenheimer (Born and Oppenheimer, 1927) approximation no longer holds. The challenge was successfully overcome for the C( 3 P)+He two-atomic system : the excellent agreement between experimental results and theory allowed a detailed description of resonance features by theory to be obtained. The situation was quite more complex for the C( 3 P)+H 2 three-atomic system , where multiple diabatic potential energy surfaces (PESs) along with spin-orbit and non-adiabatic couplings are necessary to describe its dynamics. A good agreement was also found, not sufficient however to allow for a clear assignment of resonances involving too great of a number of partial waves. Moreover, at higher collision energies, an intersystem crossing may occur with the PESs emerging from the C( 1 D)+H 2 insertion reaction. In the energy regions close to the intersystem crossing, one can expect, that the use of only triplet PESs will be too approximate to describe the collisional excitation of the C atom, which was not investigated in the study of C+H 2 collisions . Moreover, most recently, Shen et al. (2017) elucidated importance of the stationary points, in particular the so-called van der Waals saddles in the entrance channel region of the C( 1 D)-H 2 reaction. Therefore, it is also of interest to confirm the characterization of the entrance channel in the C( 3 P)-H 2 system. Our experiments will allow to test the C( 3 P)-H 2 PESs in the lower region of collision energies.
In order to get a clearer insight into the latter system, new experiments and calculations have been performed on the isotopolog system so that the C( 3 P 0 ) + D 2 → C( 3 P j ) + D 2 (with j = 1 and 2) collisional process have been studied. Measurements of state-to-state cross-sections as a function of the collision energy for C( 3 P)-D 2 scattering have been achieved, using the same apparatus as the one described in our previous studies on C( 3 P)-He (H 2 ) inelastic collisions. Quantum dynamical calculations were performed with the same PESs as for C( 3 P)-H 2 system and differing by the reactant reduced mass and rotational constant of D 2 : it thus provides a further test of these potential energy surfaces that are mandatory to accurately describe and understand the dynamics of the title system.

Experiment
Integral cross-sections were measured using a crossed beam apparatus, with variable crossing angle. The C and D 2 beams with low velocities and high velocity resolution (see Table 1) were obtained using two cryogenically cooled Even-Lavie pulsed valves (Pentlehner et al., 2009) and collided at a beam intersection angle which could be continuously varied from 90 • to 12.5 • (Chefdeville et al., 2012). C-atoms were produced by dissociation of CO diluted in neon in a dielectric barrier discharge incorporated in the faceplate of the valve (Even, 2015). ortho-D 2 (hereafter o-D 2 ) was produced after spin-conversion in a cryogenic cell by liquefaction of normal-D 2 (hereafter n-D 2 ) on NiSO 4 catalyst at low temperature (<20 K), every 45 min. The n-D 2 and o-D 2 beam velocities were changed by adjusting the temperature of the valve cold head (see Table 1 for the different experimental conditions). The collision energy, E T , in our crossed beam machine was varied by changing the angle between the two supersonic beams from χ = 90 • to 20 or 13 • : The carbon atoms were probed in their various spin-orbit states via (2+1) resonance-enhanced multiphoton ionization (REMPI) technique, using 2-photon 2p 2 3 P j → 2p3p 3 P j transitions (excitation laser tuned at 280.3 nm) at 140.149 nm, 140.157 nm and 140.170 nm for the C( 3 P 0 ), C( 3 P 1 ) and C( 3 P 2 ), respectively (Geppert et al., 2003). A third photon ionized the carbon atoms and C + is detected by a time-of-flight (TOF) mass spectrometer. Populations of ca 90-96% for C( 3 P 0 ), 4-10% for C( 3 P 1 ), and < 1% for C( 3 P 2 ) were deduced from the intensities of these transitions, consistently with previous FIGURE 1 | (3+1) REMPI spectra of n-D 2 (A) and o-D 2 (B) at crossing point for different temperature set points of the cold head. Note that for o-D 2 (B) the scale of the right part is magnified by a factor of 10. Temperatures (100, 45, and 10 K) are the set point of the cold head and correspond to the experimental conditions #2, #3, and #4 given in Table 1. studies Kłos et al., 2018). The laser beam was perpendicular to the crossing beams plane, hence avoiding any Doppler shift while scanning the crossing angle, χ, for the ICS measurements. Spectra obtained by 3+1 REMPI on the transitions C 1 u v ′ = 3, j ′ ←− X 1 + g (v ′′ = 0, j ′′ ) were employed to detect individual D 2 rotational levels (see Figure 1). Only the lowest rotational level of each nuclear spin modification, i.e., j D 2 = 0 and 1 for o-D 2 and p-D 2 , respectively, was found to be populated in the supersonic beams. The only exception was for o-D 2 , 100 K: a small signal can be seen for the R(2) transition. The ortho converted-D 2 was found to contain <6% para-D 2 . These values were found to change inappreciably over the D 2 velocities (or the temperature of the valve) and over 1.5 h.
The beam velocities and spreads ( Table 1)   . D 2 molecules in the rotational levels j = 0 and 1, were detected using the R(0) and R(1) transitions (blue circles and red diamonds); C( 3 P 2 ) atoms, produced by collisions with the D 2 beam at 70 • of the C beam were also detected (orange stars). Vertical error bars correspond to statistical uncertainties of 50 laser shots at 95% of the confidence interval. FIG, and by REMPI at the crossing point but not during the ICS measurements: it was then detected indirectly via the excited carbon C( 3 P 1 or 2 ) produced by collisions of C atoms with D 2 . In the latter case, the trigger delay of the D 2 beam for the ICS measurements was adjusted to obtain a maximum REMPI signal of carbon atoms in the ( 3 P 1 ) or ( 3 P 2 ) states. Typical REMPI profiles obtained for D 2 produced in the experimental condition #3 where the cold head temperature was set at 45 K (Table 1) are given in Figure 2. To confirm the beam profiles obtained indirectly during the ICS measurements, two other experiments were also performed independently with the REMPI technique directly on D 2 molecules (see Figure 1) or with a FIG inserted perpendicular to the molecular beam. Typical results of time-offlight (TOF) profiles are given Figure 2 for n-D 2 beam in the experimental conditions #3. All the profiles of D 2 (j D 2 = 0 and 1) may be superimposed: only the intensities differ due to the population distribution, which means that all the rotational states are generated during the expansion and uniformly spread into the beam of n-D 2 . Once the profile at the crossing point achieved, the D 2 beam arrival time, measured with the FIG at d = 393.3 mm downstream, yielded the D 2 velocity. All profiles were fitted to Gaussian functions, with peak positions t 0 and t 1 and halfwidth at 1/e (HWE), yielding the peak velocities v = d / (t 1t 0 ), and the velocity spreads δv HWE from the pulse broadening   Chefdeville et al. (2013)], and t 1 values are thus accordingly corrected. With this method, the velocities of the D 2 beam were checked, before, during and after the ICS measurements  Table 1 were determined by fitting the curves with Gaussian functions (see Figure 4).
Carbon atoms can only be detected by REMPI at the crossing point, but not with the FIG, contrarily to metastable Ne * atoms also generated within the discharge. They give a signal due to surface ionization with the FIG operated with a null filament current. Since C( 3 P) and Ne * profiles obtained by REMPI at the crossing point are very similar, it was assumed that their velocities were likely to be identical.  Again, beam profiles could also be measured at the crossing point when replacing the mass spectrometer by a FIG. The two profiles obtained for metastable Ne * are identical (see Figure 5). As for D 2 , Ne * velocity values and spreads could Frontiers in Chemistry | www.frontiersin.org be determined from profiles at the crossing point and at d = 393.3 mm downstream.
ICSs were obtained from the averaged REMPI signal intensities I REMPI and the relative velocity v r of the C and D 2 beams as I REMPI /(v r t ), where t is the mean interaction time between the two beam pulses which takes full account of the density-to-flux transformation under our working conditions (Naulin and Costes, 2014), and assuming a forward angular distribution of scattered C-atoms as for the C-H 2 system . To monitor the efficiency of the discharge, the Ne * signal from the FIG 393.3 mm downstream the crossing point was used. Moreover, the UV laser was detected by a photodiode at the entrance of the main chamber. Data points acquired with poor discharge conditions and laser power lower than 80% of the average over the whole scan were discarded. Since the densities of the two beams were not quantitatively determined, we could not extract absolute cross-sections. Relative experimental cross-sections for C( 3 P 0 ) + o-, n-D 2 → C( 3 P j=1, 2 ) + o-, n-D 2 inelastic collisions were obtained by accumulating at each angle signals from several thousand beam pulses. They were normalized by the sum of the experimental cross-sections in the energy ranges 22 −114 cm −1 for C( 3 P 0 ) → C( 3 P 1 ) transition, and 26 -165 cm −1 for C( 3 P 0 ) → C( 3 P 2 ) transition. All the plotted vertical error bars represent statistical fluctuations at a 95% confidence interval.

Theory
The full set of electronic PESs is identical for C-H 2 and C-D 2 systems and depends only on the mutual distances of the three atoms involved. Hence, in our scattering calculations of C( 3 P j ) with o-and p-D 2 we employed the most recent highly-correlated C( 3 P j )-H 2 PESs of Kłos et al. (2018) that were computed with the explicitly correlated multireference configuration interaction method (ic-MRCI-F12) Werner, 2011, 2013; with large atomic basis set. Briefly, the interaction of the open-shell C( 3 P j ) atom with the H 2 molecule gives rise to two adiabatic potentials of the A ′′ symmetry (wave function anti-symmetric with respect to the reflection in three-atomic plane) and one of A ′ symmetry (symmetric with respect to the in-plane reflection). The two adiabatic potentials were diabatized before the dynamical calculations and the diabatization procedure provided additional off-diagonal coupling. We refer the readers to Kłos et al. (2018) for more details about ab initio calculations of the PESs. The geometry of the H 2 molecule in the C-H 2 PESs is fixed at the r 0 = 0.767 Å distance corresponding to an average over the lowest vibrational state v = 0 and considered as a rigid rotor. As we substitute both H atoms with D isotopologs, we do not need to modify center of mass of the diatomic as the molecule is still homonuclear. In a case of a single isotope substitution to form an HD molecule, one would need to shift the center of mass accordingly. The rigid rotor approach for C-H 2 and C-D 2 can use the same set of rigid rotor 2-dimensional PESs assuming that we neglect any mass effects in description of H 2 and D 2 that can change slightly the equilibrium distance. The difference between vibrationally averaged distance r 0 for the D 2 molecule and H 2 molecule FIGURE 6 | Theoretical cross-sections for C( 3 P j C ) + D 2 (j D 2 ) → C( 3 P j ′ C ) + D 2 (j' D 2 ) inelastic collisions. Transitions are labeled {j D 2 j C -j' D 2 j' C }.
is only about 0.008 Å. Therefore, within these assumptions and approximations we can use our C-H 2 PESs for the C-D 2 system. To obtain integral cross-sections we solved Close-Coupling equations of Arthurs and Dalgarno (1960) using the HIBRIDON package 1 . For the C( 3 P j )-D 2 scattering we use the reduced mass of 3.0158368 a.m.u. The rotational constant of the D 2 molecule (Huber and Herzberg, 1979) is B 0 = 29.9037 cm −1 and the spinorbit energy levels of C( 3 P j ) atom (Cooksy et al., 1986;Yamamoto and Saito, 1991), listed in NIST basic atomic spectroscopic data are 0, 16.42 and 43.41cm −1 for C( 3 P 0 ), C( 3 P 1 ), and C( 3 P 2 ), respectively. The Close-Coupling equations are propagated using hybrid Alexander-Manolopoulos propagator from the initial distance of R = 1.0 to 80 a 0 . The cross-sections were checked for  Table 1); theoretical contributions of transitions C( 3 P 0 ) → C( 3 P 1 ) (blue dotted line), C( 3 P 1 ) → C( 3 P 2 ) (green dotted line), C( 3 P 1 ) → C( 3 P 0 ) (red dotted line), and total (orange solid line), assuming a 7% initial population of C( 3 P 1 ): C( 3 P 2 ) is populated by C( 3 P 0 ) → C( 3 P 1 ) (main contribution) and depopulated by C( 3 P 1 ) → C( 3 P 2 ) and C( 3 P 1 ) → C( 3 P 0 ) transitions, resulting in a total ICS tot = 0.93 σ 0−1 -0.07 (σ 1−2 + σ 1−0 ). To allow for easier comparison, experimental ICS scale is adjusted such that the area in the [22 -116] cm −1 range is the same as for the theoretical ICS calculated. Vertical error bars represent the statistical uncertainties at the 95% confidence interval; each point corresponds to 2020 (experimental conditions #1 and #4) and 1680 (experimental conditions #1 and #3) laser shots per angle, scanning the beam intersection angle between 90 • and 13 • , with −1 • decrement. The plotted error bars on energy are estimated from velocity and crossing angle uncertainties.
convergence with respect to the inclusion of a sufficient number of partial waves and energetically closed channels. The o-D 2 basis included all levels with a rotational quantum number j D 2 ≤ 6. State-to-state excitation cross-sections were obtained between all the fine-structure levels of C( 3 P) over the collision energy range relevant to the experiments (0 -800 cm −1 ) on the grid of energies with a step of 0.1 cm −1 (see Figure 6). C-H 2 and C-D 2 calculations differ by the different energy structure of the partners and by a different reduced mass.
C( 3 P 2 ) + D 2 (Figures 7-11) all exhibit a threshold behavior corresponding to the spin-orbit energy differences: E( 3 P 1 ) -E( 3 P 0 ) = 16.42 cm −1 and E( 3 P 2 ) -E( 3 P 0 ) = 43.41 cm −1 . In Figure 6 are displayed the calculated ICSs for all transitions which may contribute to the observed signals. It is worth noting that the ICSs for relaxation transitions rapidly decrease at high energies. To allow for comparison with experimental data, these ICSs were convoluted with the experimental energy resolution (Figure 12).
ICSs for involved transitions, given in the upper panels, are also displayed in the lower panels weighted by their estimated contributions to the total process: due to the presence of a small amount of C( 3 P 1 ), transitions C( 3 P 1 ) → C( 3 P 0 ) and C( 3 P 1 ) → C( 3 P 2 ) need to be taken into account. The resulting total ICS can then be compared to experimental results. For collisions with o-D 2 (Figure 7), two sets of experiments were achieved, under different D 2 -beam conditions, with different velocities: consequently, data for a given energy have been acquired at different crossing angles. The excellent agreement between both experimental sets ensures the absence of any bias in the method used to recover the ICS from the REMPI signal, which involves estimating the mean interaction time t , which depends on the crossing angle (Figure 12). Only transitions involving D 2 (j D 2 = 0) are taken into account in the overall convoluted theoretical ICS, which indeed is not the case for collisions with n-D 2 (Figure 8), where transitions involving D 2 (j D 2 = 1) also need to be taken into account with relative weights of 2/3 and 1/3, respectively.
Resonance structures observed experimentally are very similar to the theoretical ones, however slightly shifted in energy. The agreement is better for o-D 2 than for n-D 2 , since more contributions are involved in the latter case. In particular, the first two peaks at ca. 26.5 and 41.3 cm −1 for j D 2 = 0 are well resolved in both theory and experiment for o-D 2 (Figure 7A), but are blurred out by the peak at ca. 31 cm −1 for j D 2 = 1 for n-D 2 (Figure 8B). In Figure 9 are displayed partial cross sections for C( 3 P 0 ) → C( 3 P 1 ) corresponding to partial waves with total angular momenta J t from 1 to 20 that contribute within the 16-100 cm −1 total energy range. The peaks around 20 and 40 already appear at J t = 1 (thick black solid line) and are associated with opening of carbon spin orbit channels. The first lowest partial waves form sharp peaks around 20 cm −1 , whereas a broader peak around 30-40 cm −1 is due to the build-up of partial waves with J t = 8-12. The peak around 60 cm −1 comes from a shape resonance for J t = 14. A sharp shape resonance also appears for J t = 17 near 90 cm −1 .
Results for the C( 3 P 0 ) excitation by collision with o-and n-D 2 are displayed in Figures 10, 11. The convoluted theoretical ICSs for involved transitions, given in the upper panels, are also displayed in the lower panels weighted by their estimated contributions to the total process: again, due to the presence of a small amount of C( 3 P 1 ), transition C( 3 P 1 ) → C( 3 P 2 ) need to be taken into account. Note that the collisional de-excitation of C( 3 P 2 ) is not taken into account here since its initial population is negligible: furthermore, it would result in a negative offset below threshold and #3(D 2 , 45 K), in olive solid lines for #1(C) and #2(D 2 , 100 K) and in black dot lines for #1(C) and #4(D 2 , 10 K). Note that the angular spread is the main source of collision energy spread. All data are plotted as a function of the collision energy, E T . For the interaction time, a forward distribution is considered: (A) for the C( 3 P 0 ) → C( 3 P 1 ) transition and (B) for the C( 3 P 0 ) → C( 3 P 2 ) transition, same labels as for the collision energy spread.
FIGURE 13 | Integral cross sections calculated for C( 3 P 0 ) + M → C( 3 P 1 ) + M with M = He (black solid line) , p-H 2 (red solid line) , and o-D 2 (blue solid line). not observed. The resulting total ICS can then be compared to experimental results.
In both cases, two sets of experiments were achieved, under different D 2 -beam conditions, with different velocities. Whereas both experimental sets are in good agreement for o-D 2 (Figure 10B) up to 160 cm −1 , it is not the case for n-D 2 experiments. However, the beam velocity mismatch is larger for C( 3 P 0 ) → C( 3 P 2 ) experiments (v c = 815; v D2 = 845 and 1180 ms −1 , resulting in E T = 179 and 262 cm −1 at χ = 90 • ) than for C( 3 P 0 ) → C( 3 P 1 ) experiments (v c = 815; v D2 = 694 and 855 ms −1 , resulting in E T = 146 and 179 cm −1 at χ = 90 • ): at 90 • , the interaction time is much shorter than at lower angles: a variation (even small) in its estimated value can result in a larger variation of the ICS value (= I REMPI /(v r t )). It is however worth noting that the increase of the cross-section at high energies is too high to be due to a t possible underestimate. It could be due to an energy transfer involving relaxation of D 2 (j D 2 = 2 → 0): however, ICSs involving such a relaxation are monotonously decreasing (Figure 6), which would imply that their contribution should be much more intense at low energies resulting in a significant positive offset not observed. Furthermore, ICSs corresponding to rotational (de-)excitation of D 2 are weak (Figure 6). This is due to a weak anisotropy of the PES with respect to D 2 rotation that leads to a weak coupling between the D 2 rotational states. It also explains that the magnitudes of the ICSs are similar for all D 2 rotational state. In addition, the energy splitting between j D 2 = 0 and j D 2 = 2 state of D 2 is so large that the excitation probability is very small.
Another possibility to be considered is the coupling with the C( 1 D 2 ) state: its crossing with triplet PESs is estimated around 300 cm −1 by theory. Excitation to the 1 D 2 state is closed but the increase of the ICS may be due to indirect coupling that will favor the 3 P 2 state over the 3 P 1 . This would result in a decrease of the ICS for the 3 P 1 in the same energy domain (not probed in the present experiments).
The cross-sections observed are different in shape, but almost similar in average. Resonances are less visible for the C( 3 P 0 ) → C( 3 P 2 ) than for C( 3 P 0 ) → C( 3 P 1 ) ICS: actually, there are many more resonances for the 0-2 transition than for 0-1, especially for j D 2 = 1, resulting in a smoother shape. On average, their amplitudes differ by a factor of ∼2. Similar differences were found for the O-H system . The fact that the C( 3 P 0 ) -C( 3 P 2 ), C( 3 P 1 ) -C( 3 P 2 ), and C( 3 P 0 ) -C( 3 P 1 ) transitions have more of less the same magnitude may be partly explained by the huge well depth that would lead to a significant redistribution of the flux over all open C-atom spin-orbit states.

Comparison of C-D 2 With C-H 2 and C-He Systems
As shown in Figure 13, there is a great difference between C-He and C-H 2 (D 2 ) systems, due to quite different excitation processes. For C-He, the interaction is a weak van der Waals forces and the excitation is thus essentially governed by spin-orbit coupling . For C-H 2 (D 2 ), the interaction consists in a deep potential well and the system can then be chemically bound and collisional energy transfers therefore are much more efficient, as clearly shown in Figure 13. However, there is a decrease in the C( 3 P 0 ) -C( 3 P 1 ) ICSs around 50 cm −1 for all systems, essentially due to the opening of the C( 3 P 0 ) -C( 3 P 2 ) excitation. Concerning C-D 2 and C-H 2 systems, apart the resonances, ICSs are expected to be similar when no rotational (de-)excitation of H 2 (D 2 ) is involved as can be seen in Figure 13.

CONCLUSION
In this work, we have presented a joint theoretical and experimental study of the spin-orbit transitions of C( 3 P j ) by collisions with D 2 . Integral cross-sections have been experimentally observed in a crossed beam apparatus down to collision energies below ca. 5.5 cm −1 (66 J mol −1 ) and compared to state-of-the-art non-Born-Oppenheimer quantum dynamical calculations for C( 3 P 0 ) → C( 3 P 1 ) and C( 3 P 0 ) → C( 3 P 2 ) transitions. Results have been compared to similar systems previously studied (C( 3 P j ) + H 2 , and He) Kłos et al., 2018). The overall agreement obtained, in particular for C( 3 P j ) + H 2 and C( 3 P j ) + D 2 for which calculations are performed using the same potential energy surfaces, confirms the validity of these potentials which can be confidently used to compute (de-)excitation rates of Catoms in the low energy domain relevant to astrophysical modeling of cold molecular clouds. However, the present results validate the low energy data generated from theses PESs but the calculations at higher energy would require to revise the theoretical approach and probably to add the excited state of C-atom.

DATA AVAILABILITY
All datasets generated for this study are included in the manuscript and are available on request.

AUTHOR CONTRIBUTIONS
AB, SM, and CN carried out the experimental measurements and data analysis. FL and JK performed the theoretical calculations. The manuscript was written through contributions of all authors.