Photoionization Cross-Sections of Carbon-Like N⁺ Near the K-Edge (390–440 eV)

Abstract

High-resolution K-shell photoionization cross-sections for the C-like atomic nitrogen ion (N⁺) are reported in the 398 eV (31.15 Å) to 450 eV (27.55 Å) energy (wavelength) range. The results were obtained from absolute ion-yield measurements using the SOLEIL synchrotron radiation facility for spectral bandpasses of 65 meV or 250 meV. In the photon energy region 398–403 eV, $1s⟶2p$ autoionizing resonance states dominated the cross section spectrum. Analyses of the experimental profiles yielded resonance strengths and Auger widths. In the 415–440 eV photon region $1s⟶\left(1s2s^{2}2p^{2\hspace{0.17em}4}P\right)np$ and $1s⟶\left(1s2s^{2}2p^{2\hspace{0.17em}2}P\right)np$ resonances forming well-developed Rydberg series up $n=7\hspace{0.17em}\mathrm{and}n=8$, respectively, were identified in both the single and double ionization spectra. Theoretical photoionization cross-section calculations, performed using the R-matrix plus pseudo-states (RMPS) method and the multiconfiguration Dirac-Fock (MCDF) approach were bench marked against these high-resolution experimental results. Comparison of the state-of-the-art theoretical work with the experimental studies allowed the identification of new resonance features. Resonance strengths, energies and Auger widths (where available) are compared quantitatively with the theoretical values. Contributions from excited metastable states of the N⁺ ions were carefully considered throughout.

1. Introduction

X-ray spectra obtained by Chandra from sources such as Capella, Procyon, and HR 1099 provide challenges for contemporary plasma spectral modelling codes. For example, the X-ray spectrum of the bright blazar Mkn 421 observations by the Chandra LETG+HRC-S and subsequent modelling of the spectra indicated that high quality photoionization cross-section data of atomic carbon and its ions were required [1]. More recently, photoionization cross-section measurements on the atomic oxygen ion sequence [2,3,4] were used to interpret the O VI differences between satellite observations in the UV spectra of galactic and extra-galactic sight lines compared to ground based measurements made at the SOLEIL synchrotron radiation facility [5,6].

Nitrogen is ubiquitous in astrophysical environments and the sixth most populous element in the cosmos. The photoionization of atomic nitrogen species has been the subject of a number of laboratory investigations. 1s photoionization of neutral nitrogen was investigated by Stolte et al. [7] while Gharaibeh et al. measured K-shell cross-sections in N⁺ (carbon-like) [8] and N²⁺ (B-like) [9], Al-Shorman et al. investigated N³⁺ and N⁴⁺ [10]. Recently, ion yield spectra following X-ray absorption in the K threshold region of the N⁺, NH⁺, NH₂⁺ and NH₃⁺ species were obtained by Bari et al. [11]. For N⁺, these authors measured the double-ionisation yield (N³⁺) and provided resonance assignments based on both ab initio CI calculations using the General Atomic and Molecular Electronic Structure System (GAMESS) package [12] and the results of [8]. Inner-shell photoionization and Auger processes in atomic nitrogen species have also been the subject of a number of theoretical works, see for example [13,14].

In this paper, we report high resolution absolute photoionization (PI) cross-section measurements for the singly ionised carbon-like atomic nitrogen ion N⁺ over the photon energy range 398–450 eV, covering the full 1s excitation region and photon energies beyond the K-threshold. N⁺ was one of the first ions to be studied on the Multi-Analysis Ion Apparatus (MAIA) photon-ion merged-beam facility at SOLEIL [8]. This early investigation was limited to the narrow 398–406 eV photon energy range and succeeded in detecting resonance features belonging to the strongest $1s⟶2p$ excitation only. Recent substantial improvements (discussed below) to the MAIA apparatus enabled us to: (1) detect the $1s⟶2p$ resonances with much improved statistical significance leading to the observation and assignment of several additional features; (2) estimate the $1s⟶2p$ experimental Auger widths and compare with theoretical values; (3) observe and identify regular series of $1s⟶np \left(n\ge 3\right)$ resonances leading up to the K-shell ionisation limits and (4) provide improved absolute cross section measurements in both the single and double-ionisation channels.

State-of-the-art theoretical work from the Multi Configurational Dirac-Fock (MCDF) and R-matrix with pseudo-states (RMPS) methods are bench marked against these measurements. The comparison with theory allows the interpretation of resonance features found in the experimental spectra and an estimation of the metastable content of the ion beam.

2. Experimental Details

The present work was performed on the MAIA photon-ion merged-beam set-up available at the site of the SOLEIL synchrotron radiation facility [15]. MAIA allows the high-quality synchrotron photon beam to interact with a counter-propagating ion beam within a well-defined overlap region, and has been used for the last decade to investigate the relative and absolute cross section inner-shell photoionization behaviours of a range of atomic ions, see for example [16,17,18]. More recently, similar studies on molecular species were initiated, see for example [19,20,21]. Photoelectron-photo-ion coincidence studies on ionic species can also be performed with MAIA [17].

Comprehensive descriptions of the apparatus and procedures used to obtain cross-sections in free ions are available from Bizau et al. [15] and so only an outline of the main points is presented here. Molecular nitrogen was introduced into an electron cyclotron resonance (ECR) plasma source and heated by microwaves to produce ionisation. N⁺ ions, after extraction at a 4 kV voltage on the source, were selected from other multiply charged nitrogen ions by a dipole magnet and guided via an electrostatic deflector into the region of overlap with the counter-propagating monochromatized photon beam. The interaction of the synchrotron photons with the N⁺ ions resulted in the production of either N²⁺ or N³⁺ photo-ions which were separated, after exit from the interaction region, by a tuneable dipole magnet and detected by a channel plate detector. Photon energy scans of the N²⁺ and N³⁺ count rates were acquired to map out the relative single and double photoionization cross section behaviours, respectively. Absolute measurements of the N²⁺ and N³⁺ photon yield cross-section values were also carried out at a number of photon energies.

In a merged-beam experiment the ionisation cross section value $\mathsf{\sigma }\left(E\right)$ is obtained from:

$$\mathsf{\sigma }\left(E\right)=\frac{S\left(E\right)e^2\eta vq}{IJϵ{{\displaystyle \int }}_0^L\frac{dz}{\mathsf{\Delta }x\mathsf{\Delta }yF\left(z\right)}},$$

(1)

where $S\left(E\right)$ is the counting rate of the photo-ions produced by the synchrotron photons of energy $E$, $e$ is the electron charge, $\eta$ is the efficiency of the photodiode used to characterise the photon beam, $v$ is the velocity of the ions in the interaction region due to the extracting voltage, $q$ is the charge on the ion, $I$ is the current produced by the calibrated photodiode, $J$ is the ion current, $ϵ$ is the efficiency of the channel plates used to measure the photo-ions and the integral takes account of the beam overlap geometry with $z$ which defines the ion beam propagation direction.

Table 1. Values of experimental parameters used to evaluate the absolute photoionization cross-section at 400 eV photon energy.

Experimental Parameter	Value
Photo-ion counting rate $S$ (s−1)	1030
Noise (s−1)	60
Ion beam velocity $v$ (ms−1)	$2.1\times {10}^5$
Photon brilliance (photons/0.1%BP)	$6\times {10}^{12}$
Ion current $J$ (nA)	80
Channel plates efficiency $ϵ$	0.55
Form factor $F_{xy}$	13

provides a summary of the experimental parameters for the present experiments under the experimental conditions prevailing during the measurement of the absolute cross section near the maximum of the strongest resonance at 400 eV. The aforementioned experimental developments included an increased photon flux and an improved understanding and calibration of the merged beam configuration. The ion current $J$ has doubled and the reduced form factor $F_{xy}$ reflects a tighter and better-defined interaction region. Most significantly, the signal-to-noise ratio for the experiment has been very much improved. Finally, of most significance for the absolute cross section measurements, a new ion detector involving focusing optics now ensures maximum collection efficiency of the photo-ions produced due to photoionization in the merged beam overlap region. Comparison with Gharaibeh et al. [8] shows a substantial gain in overall performance and sensitivity due to the significant improvement of key experimental parameters. This is the justification for the revised cross-sectional values presented in the current work.

Photon energies were determined by calibrating with the well-known $1s⟶{\mathsf{\pi }}^{*}$ and $2p⟶3d$ transitions in N₂ [22] and Ar [23] gas, respectively, corrected for the Doppler shift resulting from the velocity of the N⁺ ions. The estimated energy uncertainty is 60 meV. Different photon energy bandpasses were used depending on the spectral region under investigation. For the strongest resonances in the 400 eV region a minimum photon bandpass of 65 meV was used for optimum spectral resolution, whereas for the higher lying resonances (425–450 eV) a mean energy bandpass of 225 meV was used. When carrying out measurements of the cross sections on an absolute basis a bandpass of 280 meV was used. We estimate the total relative experimental uncertainty in the absolute values of the cross sections to be no greater than 15%.

A complication in the interpretation of the MAIA experimental measurements may arise due to the possible presence in the overlap region of ions in long-lived metastable states that have remained populated during the journey from the ECR plasma source (this is the case for the present N⁺ experiment). The measured photo-ion spectra thus comprise ground and metastable initial states contributions, the relative strength of which depends in a non-trivial manner on the source (ECR plasma) conditions prevailing at extraction. Detailed comparisons between theoretical and experimental results can be used effectively to estimate the metastable fraction, e.g., [24].

3. Theory

3.1. Relevant Decay Processes

Photon inner-shell excitation of a N⁺ ion in either the ground or metastable states produces highly energetic 1s hole states that may decay via autoionization (resonant Auger process), forming a stable N²⁺ ion and releasing a free electron. From the initial $1s^{2}2s^{2}2p^{2 3}{P}_{0,1,2}$ ground levels of N⁺, $1s⟶np$ photo-excitation processes ($n\ge 2$) produce $1s2s^{2}2p^3{}^{3}S,{}^{3}P,{}^{3}D$ $\left(n=2\right)$ or $\left(1s2s^{2}2p^{2\hspace{0.17em}4,2}P\right)np$ ${\hspace{0.17em}}^{3}S, { }^{3}P, { }^{3}D$ $\left(n>2\right)$ inner-shell states that autoionize into the ($1s^{2}2s^{2}2p{ }^{2}P$+$ϵs_{1/2}$) or ($1s^{2}2s^{2}2p{ }^{2}D$+$ϵd_{3/2,5/2}$) continua (channels) by Coulomb interactions, according to the $\mathsf{\Delta }S=\mathsf{\Delta }L=\mathsf{\Delta }J=0$ $LS$ coupling selection rules, leaving the ion in the ground state configuration of N²⁺. This decay scheme corresponds to the $K{L}_{2,3}{L}_{2,3}$ Auger process. Other Auger processes, namely $K{L}_1{L}_1$ or $K{L}_1{L}_{2,3}$ are possible that would leave the ion in the core-excited configurations $1s^{2}2p^3$ or $1s^{2}2s2p^2$. More final state channels are open if the $1s$ electron is excited to $3p$ (higher $np$) states for the $3p$ (higher $np$) electron can now either participate or spectate in the Auger process [1] with the final core state configurations $\left(1s^{2}2s2p^2\right)$, $\left(1s^{2}2s^{2}2p\right)$ or $\left(1s^{2}2s^{2}3p\right)$, $\left(1s^{2}2s2p3p\right)$, $\left(1s^{2}2p^{2}3p\right)$, respectively, e.g., [25].

As noted earlier, the measured cross section data may be complicated by the presence of metastable states in the sample ion beam. Theoretical interpretation, thus, requires the computation of all the PI cross-sections from the relevant initially populated states that contribute. In the present case, these are $1s^{2}2s^{2}2p^2{}^1{D}_2$ (1.90 eV),${}^1{S}_0$(4.05 eV) and $1s^{2}2s2p^3{}^5{S}_2$(5.80 eV), which all lie within a few eV above the ground state [26]. The $1s^{2}2s2p^3$ ${}^5{S}_2$state is radiatively coupled to the $1s^{2}2s^{2}2p^2{}^3{P}_{1,2}$ ground $J$-levels with a total lifetime of 5.6 ms [27]. This time is sufficiently long for the initially extracted ions excited in the $1s^{2}2s^{2}2p^2{}^3{P}_{1,2}$ states to reach the interaction zone in our apparatus. Following $1s⟶np$ ($n\ge 2$) photo-excitation of $1s^{2}2s2p^3{}^5{S}_2$, autoionization decay processes such as N⁺ $1s2s\left(2p^{3\hspace{0.17em}3}P\right)n{p}^{\hspace{1em}5}P$ $⟶$ N²⁺ $1s^{2}2s2p^2$ ${}^{4}P$+$ϵs_{1/2}$ are allowed and similarly for $1s⟶np$($n\ge 2$) excitations in the $1s^{2}2s^{2}2p^2{}^1{D}_2$ and ${}^1{S}_0$ metastable states.

This brief analysis shows that the strength of the signal measured in this work in the single-ionization channel (N²⁺), at a given photon energy, will comprise simultaneous contributions from a variety of possible Auger decay processes involving several initial state channels. Theoretical modelling comprising the most important of these channels is necessary for the interpretation of the experimental data.

Further ionisation may also result from the initial X-ray absorption. The N³⁺ $1s^{2}2s^{21}S$ state lies about 77.0 eV [26] above the N⁺ $1s^{2}2s^{2}2p^{23}P$ ground state and, thus, double-photoionization processes are, in principle, energetically possible following K-shell excitation in N⁺. Double-Auger decay, Auger cascade and electron shake-off are possible atomic processes that may contribute to double-ionization in the present case. For some of the final state configurations mentioned above, e.g., $1s^{2}2p^3,$the Auger decay of the $2s$ vacancy is not energetically possible, thus preventing the Auger cascade, and return to ground state is necessarily via radiative transitions.

A schematic energy level diagram showing the main excitation and decay processes involved in this work is shown in Figure 1. It is notable that the photon-excited states include several open shells and sub-shells. This makes the problem of accurate atomic structure calculations a very demanding one, e.g., [28], and the case of N⁺ provides a particularly challenging test case for theoretical models. We have carried through extensive calculations using two different theoretical approaches, namely Multi-Configuration Dirac-Fock (MCDF) and R-matrix with Pseudo-States (RMPS) in order to evaluate their predictions compared with experiment and to help in the interpretation of the results.

3.2. Multi-Configuration Dirac-Fock (MCDF)

Multi-configuration Dirac-Fock (MCDF) calculations, based on a full intermediate coupling scheme in a jj-basis, have been performed using a recent version of the code originally developed by Bruneau [29]. The N⁺ $\left(Z=7\right)$ photoexcitation and photoionization cross-sections were computed in the Babushkin (velocity) gauge [30] in the photon energy region of the K-edge. Calculations were restricted to electric-dipole (E₁) transitions. The concept of the Slater transition state [31] was used to optimize the one-electron wave functions. Photoexcitation and photoionization cross-sections were evaluated for the five J-levels (${}^3{P}_{0,1,2}$ and ${}^1{S}_0$) of the ground configuration $1s^{2}2s^{2}2p^2$ and the ${}^5{S}_2$ lowest level of the $1s^{2}2s2p^3$ configuration. The $1s^{2}2s^{2}2pnp$ and $1s^{2}2p^{3}np$ $\left(n=3-5\right)$ configurations were added to optimize the initial state description. Photo-excited levels with $J=0,1,2$ were obtained based on the mixing of the $1s2s^{2}2p^3$, $1s2s^{2}2p^{2}np\hspace{0.17em}\left(n=3-5\right)$, $1s2p^5$, $1s2p^{4}np,n=3-5$ and $1s2s2p^4$, $1s2s2p^{3}np, n=3-5$, odd and even parity configurations, respectively. With a view to optimise eigenenergies, different radial functions for the $n{p}_{1/2,3/2}$ ($n=2-5$) orbitals were used in the initial and final configurations. The individual photoexcitation cross-sectional profiles were obtained by dressing each E₁ transition with a Lorentzian line shape of full width at half maximum (FWHM) equal to 92.4 meV to represent the Auger width. The latter value was obtained from MCDF calculations performed to calculate the statistical average of the autoionization rates from the $1s2s^{2}2p^3$ configuration to the $1s^{2}2s^{2}2p$, $1s^{2}2s2p^2$ and $1s^{2}2p^3$ configurations, respectively. The same value of 92.4 meV was used for all the members along the aforementioned Rydberg series. Continuum photoionization cross-sections were calculated using the reduced set of the $1s^{2}2s^{2}2p^2$, $1s^{2}2s2p^3$, $1s2s^{2}2p^2$ and $1s2s2p^3$ configurations.

Additionally, we note the work of Hasoǧlu et al. [32] who used multiconfiguration Dirac-Fock (MCDF) and Breit-Pauli (MCBP) theoretical methodologies to calculate the K-shell Auger and radiative decay rates of the ten possible $1s^{2}2s^{2}2p^3$ ${}^{2S+1}{L}_J$ states along the iso-electronic sequence from $Z=6$ to $Z=30$, showing the importance of both electron-electron correlation and relativistic effects even at low $Z$. Some of the Auger rates obtained by Hasoǧlu et al. [32] for $Z=7$ are amenable to direct comparison with the present experimental values (see Section 4.1).

3.3. R-Matrix (RMPS)

The photon energy range of the photoionization (PI) cross-sections presented in [8] has been extended up to 440 eV to include the K-edge region. All PI cross sections were determined using the RMPS method [33,34,35] in LS—coupling with the parallel version [36] of the programs [34,35,37]. The same 390-level model for the N²⁺ residual ion was used in the present close-coupling PI cross-section calculations as in the work of Gharaibeh et al. [8]. The RMPS resonance parameters were determined using the multi-channel R-matrix QB technique (applicable to atomic and molecular complexes) of Berrington and co- workers [38], Quigley et al. [39] and Ballance et al. [40]. The resonance width $\mathsf{\Gamma }$ may be determined from the inverse of the energy derivative of the eigenphase sum $\delta$ at the position of the resonance energy $E_r$ via:

$$\mathsf{\Gamma }=2{\left[\frac{d\delta }{dE}\right]}_{E=E_r}^{-1}=2{\left[{\delta }^{\prime }\right]}_{E=E_r}^{-1},$$

(2)

Further relevant theoretical details can be found in Gharaibeh et al. [8].

4. Results and Analyses

The experimental results are presented in Figure 2 showing the measured cross-sections for single and double photo-ionization of N⁺ in the 398–450 eV photon energy region. The photon energies at which absolute measurements were carried out are indicated. Both spectra feature a strong discrete resonance region in the 399–405 eV photon range which corresponds with the decay of N⁺ ions following $1s⟶2p$ electron excitation. The four main peaks observed in the single ionization channel are seen to have counterparts in the double-ionization channel at the same photon energies. Additional, previously unobserved, resonance features appear in the 415–440 eV photon energy region in both the single and double ionisation channels. This is the region corresponding to the decay of N⁺ ions following $1s⟶np$ excitations with $n\ge 3$. Some resonances are seen to form distinctive Rydberg series, particularly in the double-ionization channel, while continuum processes begin to contribute significantly to the cross-section upward of ~430 eV photon energy. Resonance series due to $1s⟶np$ excitations in the ${\hspace{0.17em}}^{1}P{,}^{1}D$ and ${\hspace{0.17em}}^{1}S$ initial states converge to the $1s2s^2{\left(2p^{23}P\right)}^{4,2}P$, $1s2s^2{\left(2p^{21}D\right)}^{2}D$ and $1s2s^2{\left(2p^{21}S\right)}^{2}S$ inner ionisation limits in N²⁺, respectively. Excitations from the $1s^{2}2s2p^{35}S$ state will result in additional limits. Detailed analyses for the two photon regions 398–403 eV ($1s⟶2p$) and 415–450 eV ($1s⟶np,n\ge 3$) are given below in the light of the MCDF and RMPS theoretical results.

4.1. 1s → 2p Resonances

Figure 3 shows the ab initio results of our RMPS and MCDF total photoionization cross-section calculations for the resonances in the 398–404 eV region. These arise from the photon excitation of an inner shell 1s electron to a 2p valence shell, starting from the assumed initial levels $1s^{2}2s^{2}2p^{23}{P}_{0,1,2}{,}^1{D}_2{,}^1{S}_0$ and $1s^{2}2s2p^{35}{S}_2$. Figure 4a shows a high-resolution experimental single-ionisation spectrum (65 meV band pass) in the same region which clearly reveals additional resonances not reported by Gharaibeh et al. [8]. The resonance features in Figure 4a are assigned the numerical labels that are used in

Table 2. Experimentally determined atomic parameters (energy, Auger width and oscillator strength) of the main $1s⟶2p$ resonances (~400 eV photon energy) in the N⁺ photoionization cross-section spectrum, estimated from the absolute measurements of single-ionisation yields and comparison with theoretical values.

Resonance #Label	Measured Energy a (eV)	RMPS Energy (eV)	MCDF Energy (eV)	Experimental Width a,b (meV)	RMPS Width (meV)	MCBP/ MCDF Width (meV) [32]	Measured Strength a,c (MbeV)	Scaled Strength d,e (MbeV)	RMPS Strength f (MbeV) This Work	MCDF Strength g (MbeV) This Work
1	399.840(2)	399.709	399.275	73(11)	124	171/181	5.7(1.8)	7.6	10.1	14.5
2	399.994(26)	399.891	400.488	167(70)	62		1.4(8)	34.1	16.2	22.9
x	x	400.159	399.98		115				24.6	27.2
3	400.728(2)	400.579	400.094	79(9)	78	33/79	8.6(2.5)	11.5	6.8	9.8
4	400.862(9)	400.681	400.199	116(24)	105		2.9(1.0)	14.9	18.0	26.8
5	401.397(2)	401.347	400.507	70(10)	121	145/148	3.5(1.0)	4.7	6.3	9.0
6	402.378(14)	402.320	401.439	128(48)	132		1.0(0.4)	5.1	6.4	8.4

^a The number in brackets is the numerical uncertainty on the last digit, i.e., 399.840(2) eV means 399.840 ± 0.002 eV obtained from a Voigt profile deconvolution of the experimental line shape (peak energy position and width). The overall energy uncertainly must also include the 60 meV energy calibration contribution (see text). ^b This is the Lorentzian width obtained from a Voigt profile deconvolution of the experimental line shape. ^c Obtained from a numerical integration of the measured line profile. ^d Obtained assuming 0.748 ³P + 0.194 ¹D + 0.016 ¹S + 0.041 ⁵S initial states contributions (see text). The numbers in this column are comparable with the theoretical RMPS and MCDF strengths. ^e Total strength of 83.2 Mb eV. ^f Total strength of 88.41 Mb eV. ^g Total strength of 118.6 Mb eV.

, which provides the resonance identifications and atomic parameters. Figure 4a also shows the results of Voigt profile numerical deconvolutions of the measured lineshapes.

The $1s^{2}2s^{2}2p^{23}{P}_1$ and $1s^{2}2s^{2}2p^{23}{P}_2$ states lie 6.04 meV and 16.22 meV, respectively above the $1s^{2}2s^{2}2p^{23}{P}_0$ ground state. Such small energy differences are not amenable to discrimination in the present experimental conditions and we, thus, consider initial excitations from these three levels proportionally to their statistical weight. For the sake of simplifying the notation, we shall also generally omit the $J$-value in the notation of the relevant $\left(LSJ\right)$ states in the rest of the paper. From Figure 3, both theoretical approaches predict three strong resonances originating from the ${\hspace{0.17em}}^{3}P$ ground state to the $1s2s^{2}2p^{33}D{,}^{3}S\mathrm{and}{}^{3}P$ states (in increasing order of energy). The strong experimental resonances 1, 3 and 5 in Figure 4a measured at 399.84 eV, 400.73 eV and 401.40 eV, respectively, are readily assigned to these transitions, respectively. The ab initio energies predicted by the MCDF (RMPS) theories are 399.28 (399.709) eV, 400.48 (400.579) eV and 400.53 (401.347) eV, corresponding to experimental vs. calculated energy differences of 0.56 (0.131) eV, 0.25 (0.149) eV and 0.87 (0.05) eV, for the same transitions, respectively. This comparison shows that the RMPS theory, as implemented in the manner described in Section 3, more accurately predicts the experimental values than the MCDF results which show differences of 0.25 eV or greater.

From the theoretical results of Figure 3, it is reasonable to assign the isolated resonance peak 6 observed at 402.36 eV to the $1s^{2}2s^{2}2p^{21}D⟶1s^{2}2s2p^{31}P$ transition (Table 2). It follows that the deconvolved shoulder at 400.85 eV, resonance 4 in Figure 4a, can be attributed to the $1s^{2}2s^{2}2p^{21}D⟶1s2s^{2}2p^{31}D$ transition. RMPS theory results for the resonance energies are again in closer agreement with experiment than the MCDF values (Table 2). Nevertheless, both theoretical approaches agree on these assignments.

Figure 4a shows a remaining (deconvolved) resonance 2 at 399.994 eV in the high-energy shoulder of the ${\hspace{0.17em}}^{3}P\hspace{0.17em}⟶{}^{3}D$ peak. Figure 3 shows the MCDF and RMPS predictions for transitions arising from the excited states $1s^{2}2s^{2}2p^{21}S$ and $1s^{2}2s2p^{35}S$ and differences exist here between the two theoretical approaches. MCDF suggests resonance 2 to be the $1s^{2}2s^{2}2p^{21}S⟶1s2s^{2}2p^{31}P$ transition. RMPS suggests instead that this is a contribution from the $1s^{2}2s2p^{35}S⟶1s2s2p^{45}P$ transition, theoretically predicted at 399.89 eV and closely matching the experimental resonance at 399.98 eV. Taking into account the generally very good agreement between the RMPS predicted energies and experimental values, we assign resonance 2 to the ${\hspace{0.17em}}^{5}S\hspace{0.17em}⟶{\hspace{0.17em}}^{5}P$ transition. We note further corroborating evidence for this assignment when the next member of the Rydberg series, for which resonance 2 in Table 2 is the first member, is unequivocally identified (the next member in question is resonance 1 in Table 5 of Section 4 below).

To provide a fuller comparison with experiment the ab initio MCDF and RMPS results of Figure 3 were convolved with Gaussian profiles of 65 meV FWHM to simulate the experimental broadening. The theoretical cross-section values, corresponding to the ground and excited state initial configurations, were weighted by numerical factors representing the relative populations of the initial states. The results are shown in Figure 4c,d. It is clear that the dominant initial configuration is the ground state ${\hspace{0.17em}}^{3}P$, with smaller contributions from the ${\hspace{0.17em}}^{1}D$ and ${\hspace{0.17em}}^{5}S$ states. The ratios of the measured to the calculated cross-section values can provide an estimate of the initial state fractions. The sum of the integrated experimental intensities (single-ionisation channel only) of the resonances originating in the ${}^{3}P$ state is 6.0 + 9.1 + 3.7 = 18.8 MbeV, while for the RMPS predictions it is 10.1 + 6.8 + 6.3 = 23.2 MbeV, providing a ratio of 0.81 (Table 2). For the ${\hspace{0.17em}}^{1}D$ resonances, the numbers are 3.90 MbeV and 24.4 MbeV, respectively, with a ratio of 0.16, while for the ${\hspace{0.17em}}^{5}S$ ones the ratio would be $1.4/16.2\approx 0.09$. We note that these relative population values are quite close to those obtained for a Maxwell-Boltzmann equilibrium at a temperature of ~2.5 eV, for which the weighting factors would be 0.75 ${\hspace{0.17em}}^{3}P$, 0.19 ${\hspace{0.17em}}^{1}D$, 0.016 ${\hspace{0.17em}}^{1}S$ and 0.04 $\hspace{0.17em}{\hspace{0.17em}}^{5}S$. This agreement may be somewhat fortuitous as it it realised that temperature may not be a meaningful physical concept in this case. However, such factors can be appropriately used to model theoretical cross-sections against experimental ones. Furthermore, the error bars on the experimental/theoretical cross-section ratios are large and include the relative error on the experimental integrated intensities of at least 10% (Table 2) and the contributions to the total cross-section due to the double-ionization channel. Figure 2 shows that the double ionization channel does contribute markedly in the 400 eV region with an estimated contribution of about 5%.

In Figure 4, we scale the theoretical cross-sections by factors of 0.75 ${\hspace{0.17em}}^{3}P$, 0.19 ${\hspace{0.17em}}^{1}D$, 0.016 $\hspace{0.17em}{\hspace{0.17em}}^{1}S$ and 0.04 ${\hspace{0.17em}}^{5}S$ to allow direct comparison with the experiment. The summed results are displayed in Figure 4c,d. From Figure 4, we conclude that the above analyses lead to an overall satisfactory agreement between the MCDF and RMPS theories and experiment in respect of the resonance strengths and energy positions. The RMPS results in Figure 4d reproduce well the experimental observations of Figure 4a in terms of resonance positions and relative intensities, whereas the MCDF peak absolute cross sections seem in better agreement with the experimental values. The very weak feature at 400.16 eV in the RMPS modelled spectrum is associated with the ${\hspace{0.17em}}^{1}S⟶{}^{1}P$ transition (labelled x in Table 2 and

Table 3. Resonance Assignments near 400 eV photon energy.

Resonance #Label 1	Transition
1	$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶1s2s^{2}2p^{3\hspace{0.17em}3}D$
2	$1s^{2}2s2p^{3\hspace{0.17em}5}S⟶1s2s2p^{4\hspace{0.17em}5}P$
x	$1s^{2}2s^{2}2p^{2\hspace{0.17em}1}S⟶1s2s^{2}2p^{3\hspace{0.17em}1}P$
3	$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶1s2s^{2}2p^{3\hspace{0.17em}3}S$
4	$1s^{2}2s^{2}2p^{2\hspace{0.17em}1}D⟶1s2s^{2}2p^{3\hspace{0.17em}1}D$
5	$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶1s2s^{2}2p^{3\hspace{0.17em}3}P$
6	$1s^{2}2s^{2}2p^{2\hspace{0.17em}1}D⟶1s2s^{2}2p^{3\hspace{0.17em}1}P$

¹ Same as Figure 4 and Table 2.

). The noise present in the measured data in this region together with an estimated very low scaling factor for ${\hspace{0.17em}}^{1}S$ prevent definite confirmation.

All the results from the RMPS and MCDF calculations in terms of energies (eV) and line strengths (Mb eV) are presented in Table 2 and compared with the experimental measurements. Table 2 also includes the measured line widths (meV) obtained from a Voigt profile numerical deconvolution of the experimental resonance shapes. This allows removal of the 65 meV FWHM Gaussian instrumental broadening from the measured total line width with the remaining Lorentzian FWHM representing mostly the Auger width of the final state of the resonance. The RMPS resonance widths (see Section 3) either match quite well (${\hspace{0.17em}}^{3}S$,${\hspace{0.17em}}^{1}D$,${\hspace{0.17em}}^{1}P$) or differ by no more than a factor of about two (${\hspace{0.17em}}^{3}D$,${\hspace{0.17em}}^{5}P$,${\hspace{0.17em}}^{3}P$) from the measured widths, taking into account the relative uncertainties from ~15% up to ~40%.

Inter-comparing the integrated intensities (resonance strengths) of the resonances originating from the same initial $LS$ term allows a relative comparison with theory independent of the initial population fractions. The ${\hspace{0.17em}}^{3}P⟶{}^{3}D$, ${\hspace{0.17em}}^{3}P⟶{}^{3}S$ and ${\hspace{0.17em}}^{3}P⟶{}^{3}P$ intensities are observed in the ratios of 1/1.5/0.6. This is to be compared to the ratio of 1/0.7/0.6 predicted by both the RMPS and MCDF theories. Agreement between experiment and the RMPS and MCDF theories is, thus, reasonably close, although for both theories this is less satisfactory for the ${\hspace{0.17em}}^3{S}_1$ state. Hasoğlu et al. [32] discussed how peculiar spin-orbit mixing effects with ${\hspace{0.17em}}^3{P}_1$ affect the Auger and radiative rates of the ${\hspace{0.17em}}^3{S}_1$ state along the $1s2s^{2}2p^3$ isoelectronic sequence. However, the authors show these effects peak around $Z=17$ nuclear charge and play only a small part in the present case of $Z=7$ nuclear charge. For the resonances originating in the $1s^{2}2s^{2}2p^{21}{D}_2$ excited state, the 1/0.36 $\left({\hspace{0.17em}}^{1}D⟶{}^{1}D{/}^{1}D⟶{}^{1}P\right)$ experimental ratio is well reproduced by both the MCDF and RMPS theories. The total integrated experimental intensities of the six identified resonances, assuming the aforementioned initial state fractions, amounts to (83 ± 12) Mb eV, which is equivalent to a discrete oscillator strength of 0.76 ± 0.15 [41]. These figures compare very favourably with the theoretical RMPS values of 88.4 MbeV and 0.80, respectively, while the MCDF values of 118.6 MbeV and 1.1 are somewhat overestimated.

We have already mentioned the sizeable contribution (~5%) to the total cross section of decay processes leading to double ionisation of the final product (N³⁺). We see from Figure 3b that in the 400 eV region of $1s⟶2p$ excitations, the resonances structure for the doubly-ionisation spectrum is almost exactly coincident in energy and relative intensity with that in the single ionisation channel. This suggests the double-Auger process for the double-ionisation channel, whereby the $1s2s^{2}2p^3$ inner-shell excited configuration non-radiatively decays to the final $1s^{2}2s^2$ configuration of N³⁺ (Auger cascade is not possible here) with a $2p$ electron filling the initial $1s$ hole and the other two highly correlated $2p$ electrons being simultaneously ejected.

The N³⁺ ion yield data of Bari et al. [11] in the 400 eV region are in reasonable agreement with the present data of Figure 4b for both the main resonances energies and relative intensities. However, resonance assignments suggested by Bari et al. [11], based on their own GAMESS configuration interaction (CI) calculations and the previous work of Garabeih et al. [8], differ to some extent from those provided by the detailed analyses of the present work. The more complete comparisons shown between the present absolute measurements (see Section 2) and the results of extended atomic structure calculations from two theoretical approaches lead us to believe that the revised analyses of the present work are conclusive.

4.2. 1s → np (n ≥ 3) Resonances

Excitation of a $1s$ electron into $np\hspace{0.17em}\left(n\ge 3\right)$ subshells from a ${\hspace{0.17em}}^{3}P$ ground state N⁺ ion, leads to the two main series: $1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P\hspace{0.17em}⟶\left(1s2s^{2}2p^{2\hspace{0.17em}4}P\right)n{p}_{1/2,3/2}{\hspace{0.17em}}^{3}S,{}^{3}P{,}^{3}D$ and $1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶$ $\left(1s2s^{2}2p^{2\hspace{0.17em}2}P\right)n{p}_{1/2,3/2}{\hspace{0.17em}}^{3}S,{}^{3}P{,}^{3}D$ converging to the $1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{\hspace{0.17em}4}P$ and $1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{\hspace{0.17em}2}P$ inner-shell limits, respectively. Additionally, if $1s$ excitations from the ${\hspace{0.17em}}^{1}D$,${\hspace{0.17em}}^{1}S$and ${\hspace{0.17em}}^{5}S$ excited states have contributions, then we obtain several additional series converging on the $1s2s^2{\left(2p^{2\hspace{0.17em}1}D\right)}^{\hspace{0.17em}2}D$, $1s2s^2{\left(2p^{2\hspace{0.17em}1}S\right)}^{\hspace{0.17em}2}S$ and $1s2s{\left(2p^{3\hspace{0.17em}4}S\right)}^{\hspace{0.17em}6}S$ limits, respectively. The contributions of the latter two to the measured total cross-sections are necessarily reduced compared to the ground state contributions as a result of the increasingly lower high n resonance strength coupled to the smaller fractional population factors established in the previous section. The RMPS and MCDF calculated series limits are shown in

Table 4. RMPS, MCDF and experimental (see text) N³⁺ series limits (eV).

Main 1s Limits in N3+	RMPS	MCDF	EXPT
$1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{\hspace{0.17em}4}P$	431.06	431.8	431.49
$1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{\hspace{0.17em}2}P$	436.23	435.49	436.32
$1s2s^2{\left(2p^{2\hspace{0.17em}1}D\right)}^{\hspace{0.17em}2}D$	435.57	435.51	1
$1s2s^2{\left(2p^{2\hspace{0.17em}1}S\right)}^{\hspace{0.17em}2}S$	438.20	439.20	1

¹ No measurements.

. No limits are calculated for the atomic states based on the $1s2s2p^3$ configuration.

In Figure 5, we show the ab initio MCDF and RMPS theoretical predictions for the higher energy range of 415–440 eV. These, together with those of Table 4 and

Table 5. Experimentally determined energy and strength of the main $1s⟶np,n\ge 3$ resonances (415–440 eV photon energy) in the N⁺ photoionization cross-section spectrum, estimated from the absolute measurements of single-ionisation and double-ionization yields and comparison with theoretical energy values.

Resonance #Label See Figure 5c	Single Ionization (SI) Channel Energy a (eV)	SI Channel Resonance Strength b (MbeV)	Double Ionization (DI) Channel Energy a (eV)	DI Channel Resonance Strength b (MbeV)	RMPS Photon Energy (eV)	MCDF Photon Energy c (eV)	Assignment
1	418.53(3)	0.16	418.53(3)	0.03(1)	418.26	419.14	$1s^{2}2s2p^{35}S⟶1s2s2p^{3}3p{ }^{5}P$
2	421.74(3)	0.3(1)	421.76(4)	0.03	421.97	421.96	$1s^{2}2s^{2}2p^{23}P⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{4}P\right]3p^{{\hspace{0.17em}}^3}S$
3 d	422.25(13)
4	422.61(2)	1.3(6)	422.66(3)	0.4(1)	422.55	422.66	$1s^{2}2s^{2}2p^{23}P⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{4}P\right]3p^{{\hspace{0.17em}}^3}D$
5	422.96(7)	0.5(4)	422.97(1)	0.22(6)	422.84	422.95	$1s^{2}2s^{2}2p^{23}P⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{4}P\right]3p^{{\hspace{0.17em}}^3}P$
6 d	424.13		424.13
7	424.55	0.6(2)	424.55	0.37(3)	424.78	424.30	$1s^{2}2s^{2}2p^{2\hspace{0.17em}1}D⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}1}D\right)}^{2}D\right]3p^{\hspace{0.17em}1}L$
8			425.99				$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶\left[1s2s^{2}2p^2\right]3p^{\hspace{0.17em}3}L$
9 d	426.6		426.60
10	426.88(1)	1.6(3)			426.97	426.66	$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{4}P\right]4p$
10			426.92(1)	0.76(3)		426.78	$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{2}P\right]3p$
11			428.74(3)	0.15	428.63	428.615	$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{4}P\right]5p$
12			429.07(6)	0.12	429.18	428.80	$1s^{2}2s^{2}2p^{2\hspace{0.17em}1}D⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}1}D\right)}^{2}D\right]4p$
13			429.61(2)	0.2	429.34	429.46	$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{4}P\right]6p$
14			430.20(2)	0.1			$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{4}P\right]7p$ e
15			430.81(5)	0.25	431.13	430.57	$1s^{2}2s^{2}2p^{2\hspace{0.17em}1}D⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}1}D\right)}^{2}D\right]5p$
16 d			431.56(7)	0.55
17			431.72(1)	0.45	f	431.40	$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{2}P\right]4p$
18 d			433.19
19			433.58(1)	0.26	f	433.18	$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{2}P\right]5p$
20			434.41	0.1	f	434.09	$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{2}P\right]6p$
21			434.93	0.11			$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{2}P\right]7p$ e
22			435.32				$1s^{2}2s^{2}2p^{2\hspace{0.17em}3}P⟶\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{2}P\right]8p$ e
23 d			435.63
24 d			435.95

^a Peak energy value obtained from a Voigt profile deconvolution of the experimental line shape. The number in brackets is the numerical uncertainty on the last digit. The overall energy uncertainly must also include the 60 meV energy calibration contribution (see text). ^b Obtained from a numerical integration of the measured line profile. The number in brackets is the numerical uncertainty on the last digit. This is at least 50% if no uncertainty value is quoted in brackets. No entry means that the error is too large for a strength value to be reliably quoted. ^c These energy values are shifted by +2.0 eV. ^d See text. ^e Assignment is based solely on Rydberg analysis of experimental energies. No theoretical RMPS or MCDF data are available. ^f RMPS energy not available.

, are used as the basis for the analyses of the experimental data presented in Figure 6. In Figure 6a, the absolute cross-sectional data for the single ionisation channel are shown. This channel contains no marked resonance contributions above noise at photon energies greater than ~427/8 eV. Resonance structure above this energy and up to ~436 eV is seen in the double ionisation, shown in Figure 6b, channel only, whereas this channel also contains resonance structures whose energies match those of the single ionisation channel in the region ~418–426 eV. The details of the resonance strengths and energy positions are given in Table 5.

These data are obtained from Voigt profile numerical fitting of the experimental resonance data profiles including a 250 meV FWHM Gaussian to simulate the energy band pass. Above 428 eV, for reasons of computational stability, Gaussian profiles only were used to extract resonance parameters. The resonances labelled #3, 6, 9, 16, 18, 23, 24 in Table 5 correspond to very low intensity features that are not readily identifiable as peaked atomic resonances, see Figure 6a,b. They arise during the experimental line fitting procedure and are the result of simulating either slightly asymmetric profiles or very weak spectral features and do not affect the general analyses of the data. As remarked earlier, the open shell nature of N⁺ means that the spectral density of resonances in this energy range is very high.

Both the RMPS and MCDF calculations confirm that the 418.58 eV resonance can only originate from the ${\hspace{0.17em}}^5{S}_2$ excited state connecting to several $1s2s2p^{3}3p\hspace{0.17em}$ final states with dominant ${\hspace{0.17em}}^{5}P$ character (this notation is adopted in Table 4). This assignment was used in Section 4.1 above to establish the assignment of the low-energy resonance (labelled 2 in Table 2 and Table 3) in the 400 eV photon region.

The strong resonances at 421.74 eV, 422.61 eV and 422.96 eV are identified as the ${\hspace{0.17em}}^{3}S,{\hspace{0.17em}}^{3}D\hspace{0.17em}\mathrm{and}{\hspace{0.17em}}^{3}P$ $LS$ components of the $\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{4}P\right]3p$ member of the low energy ${\left(2p^{2\hspace{0.17em}3}P\right)}^{4}P\hspace{0.17em}np$ Rydberg series, respectively. The corresponding single-valued theoretical energies for these and the higher Rydberg states shown in Table 4 are actually the result of the strength-averaged contributions of many mixed $LSJ$ states with $J=1\hspace{0.17em}\mathrm{or}\hspace{0.17em}2$ with almost overlapping energies. As the value of n increases, the energy differences between the (increasingly hydrogenic) $LSJ$ states are almost indistinguishable, allowing Rydberg series analysis based on quantum defect values. The relatively strong resonance (#10) is the contribution of two components at 426.88 eV and 426.91 eV, in the single and double ionisation channels respectively, with about 8 Mb total peak intensity, see Figure 6a–c. Comparison with MCDF theoretical results shows that peak #10 is the blended contribution of the $\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{4}P\right]4p$ and $\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{2}P\right]3p$ resonances. Non-linear least-square fitting of the measured photon energies $E_n$ (eV) of the resonances numbered 10 (426.88 eV), 11, 13 and 14 to the $E_n=I_p-54.42/{\left(n-\delta \right)}^2$ Rydberg formula where δ is the quantum defect and $I_p$ the ionisation energy (eV) returns best-fit values of $I_p=\left(431.49\pm 0.03\right)$ eV and δ = 0.56 ± 0.02. This value of $I_p$ is in good agreement with the RMPS and MCDF calculations and the $\delta$ value is typical for a $p$ electron orbit. These values allow the identification of the $\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{4}P\right]np$ resonances up to $n=7$. The agreement with the RMPS and MCDF calculated energies is noted. A similar approach for the resonances labelled 10 (426.91 eV), 17, 19, 20, 21 and 22 yields best-fit values of $I_p=\left(436.32\pm 0.03\right)$ eV and δ = 0.59 ± 0.01. This is in good agreement with the RMPS calculations (Table 4 and Table 5) and allows the identification of the $\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{2}P\right]np$ series up to $n=8$. Above 431.4 eV photon energy the most likely process is direct $1s$ ionisation to $1s2s^{2}2p^2$ states followed by $KLL$ Auger decay in N²⁺ leading to a continuous ion signal in the double-ionisation channel only, as observed in Figure 5b. As discussed in Section 3.1, other double-ionisation processes are conceivable for excited $1s2s^{2}2p^{2}np,\hspace{0.17em}n\ge 3$ configurations consisting of cascade or double-Auger participator and spectator decays. These processes are energetically possible below the 431.4 eV K-edge and explain satisfactorily the observations of Figure 6b. Single-electron autoionization decay of the $\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{4}P\right]3p$ and $\left[1s2s^2{\left(2p^{2\hspace{0.17em}3}P\right)}^{4}P\right]4p$ configurations are the main contributions to the single-ionisation channel as observed in Figure 6a.

Resonance #7 at 424.55 eV corresponds to transitions to $\left[1s2s^2{\left(2p^{2\hspace{0.17em}1}D\right)}^{2}D\right]3p{\hspace{0.17em}}^{1}L$ states originating in the $1s^{2}2s^{2}2p^2{\hspace{0.17em}}^1{D}_2$ metastable state with roughly equal contributions in the single and double-ionisation channels. The resonances labelled 12 and 15 measured at 429.07 eV and 430.81 eV may tentatively be assigned to the $4p$ and $5p$ members of this series, respectively. Other contributions from excited states are extremely weak and unambiguous assignments are not possible.

To allow direct comparison with the theoretical data, the single and double ionisation experimental signals are added and the result shown in Figure 6c. In Figure 6d,e, the theoretical data of Figure 5 are adjusted in the manner used and discussed in Section 4.1, i.e., 0.75${\hspace{0.17em}}^{3}P$, 0.19${\hspace{0.17em}}^{1}D$, 0.016${\hspace{0.17em}}^{1}S$ and 0.04${\hspace{0.17em}}^{5}S$ initial state weight coefficients are applied following 225 meV FWHM Gaussian convolution. The MCDF theory shows a very satisfactory agreement with the measured cross-section profile in terms of relative energy positions and absolute intensities for the high energy resonances, although the absolute resonance energies are systematically too low by about 2 eV. Conversely, the RMPS theory predicts quite accurately the measured resonance energies while the peak intensities are typically too small by a factor of 2–3.

Only a qualitative comparison of the N³⁺ ion yield data by Bari et al. [11] (their Figure 3b) is feasible. It indicates a reasonable agreement between the resonance energies and intensity patterns observed in the two works.

5. Conclusions

Enhanced experimental conditions at the MAIA crossed beam facility at SOLEIL allowed substantially improved single- and double-ionisation cross section measurements to be carried out for the N⁺ ion in the K-shell excitation regime. In addition to the strong resonances in the 398–405 eV range corresponding to $\hspace{0.17em} 1s⟶\hspace{0.17em}2p$ excitations, several well-developed Rydberg resonance series corresponding to $\hspace{0.17em} 1s⟶\hspace{0.17em}np,\hspace{0.17em}n\ge 3$ excitations were observed at higher photon energies running to K-shell ionization limits above 430 eV. With three open shells the calculation of such resonance series presents a considerable challenge to theory. Furthermore, contributions due to metastable states had also to be taken into account. Comparison of the measured results with theoretical photoionization cross-section calculations from large-scale MCDF and RMPS photoionization cross section calculations allowed interpretation of the experimental data and benchmarking of the different theoretical approaches. The present theoretical work may be incorporated into astrophysical modelling codes like CLOUDY [42,43], XSTAR [44] and AtomDB [45] used to numerically simulate the thermal and ionization structure of ionized astrophysical nebulae