Abstract
The development of theories and methods devoted to the accurate calculation of the electronic quasiparticle states and levels of molecules, clusters and solids is of prime importance to interpret the experimental data. These quantum systems are often modelled by using the Born–Oppenheimer approximation where the coupling between the electrons and vibrational modes is not fully taken into account, and the electrons are treated as pure quasiparticles. Here, we show that in small diamond cages, called diamondoids, the electron–vibration coupling leads to the breakdown of the electron quasiparticle picture. More importantly, we demonstrate that the strong electron–vibration coupling is essential to properly describe the overall lineshape of the experimental photoemission spectrum. This cannot be obtained by methods within Born–Oppenheimer approximation. Moreover, we deduce a link between the vibronic states found by our manybody perturbation theory approach and the wellknown Jahn–Teller effect.
Introduction
Molecularsized nanoparticles are applied in diverse areas of basic and applied science, from drug delivery across photovoltaics and quantum information processing, harnessing their unique response to electromagnetic fields^{2,3,4}. Understanding the electronic structure of these systems is an inevitable key step to determine their optical, magnetic and other related properties. One of the most widely used experimental techniques to measure the electronic structure of small nanoparticles and molecules is photoemission spectroscopy. The photoemission spectrum (PES) gives detailed information about the binding energy of the (valence) electrons. Nevertheless, the interpretation of the PES of molecules and nanoparticles may be not as straightforward as for atoms whose spectrum is dominated by sharp peaks^{4}. In molecules and nanoparticles, vibrations may play a major role in the ionization process resulting in broad features in PES.
The effect of vibrations in the ionization is often considered within the Born–Oppenheimer approximation where the electrons are decoupled from the vibrations and assumed to be almost perfect quasiparticles (QPs). An approach based on a manybody perturbation theory (MBPT) that goes beyond the BornOppenheimer approximation has been recently proposed^{5,6,7}. In this approach both the static and dynamical coupling between electrons and vibrational modes is considered.
Here we show by means of this MBPT approach that in small diamond cages, called diamondoids^{9,10,11}, the electron–vibration coupling leads to the breakdown of the QP picture. As a consequence, the lineshape of their experimental PES can be only reproduced by taking the resultant vibronic states into account. Our MBPT approach is able to predict the Jahn–Teller nature of the corresponding electron states even for deep energy regions. These findings demonstrate the ground breaking impact of our theory in the correct understanding of the most basic photoionization phenomenon in small carbonbased nanoclusters.
Results
Photoionization spectrum of diamondoids
We demonstrate that the interpretation of the PES of selected diamondoids^{9,12,13}, for which the experimental data are available^{14,15}, in terms of atomiclike, sharp electronic levels is bound to fail. As the geometries of these nanoobjects are exactly known, they serve as testbeds to study the accuracy of the standard theoretical tools that aim at describing, from first principles, the electronic structure. Indeed, several density functional theory (DFT)^{16,17,18}, MBPT and Quantum Monte Carlo^{19,20,21,22,23} studies have focused on understanding the optoelectronic properties of diamondoids. We consider here the smallest diamondoid with a single diamond cage, called adamantane, characterized by a T_{d} symmetry and consisting of only carbon (C) and hydrogen (H) atoms. We also study diamantane, which is composed of two diamond cages with D_{3d} symmetry, and a derivative called urotropine with T_{d} symmetry, where the C–H units of adamantane are substituted by nitrogen (N) atoms (see Fig. 1c).
The measured and calculated PES of these structures are compared in Fig. 1 at different levels of theory. We start from Kohn–Sham (KS) density functional theory within the local density approximation (LDA). Local (LDA) and other (semi)local DFT functionals provide appropriate zerothorder approximation for the ground state of the system including the singleparticle KS states and energy levels^{19,18,24}. The electron QP levels are calculated within the singleshot GWmethod. We note here that fairly convergent QP levels have been obtained for energies down to −15 eV for adamantane and urotropine, and −11 eV for diamantane^{23}. Thus, we study the corresponding PES in these photoionization energy ranges.
The effect of vibrations on the PES is treated semiclassically, without dynamical effects, and by including dynamical effects induced by the electron–vibration coupling via MBPT. In the former method, the broadening, or lineshape, of the electron QP levels is described with the Huang–Rhys (HR) method (see ‘Methods’ section and Supplementary Methods), which simulates the geometry changes induced by ionization^{14} within the Born–Oppenheimer approximation. We find that the typical total HR factor is S≈3 for the considered diamondoids (see Supplementary Fig. 1), which implies that three vibrational modes are involved in the geometry change. In the latter method, instead, the effect of vibrations on the PES is directly included in the spectral function (SF), computed within the recently implemented MBPT approach to the electron–vibration coupling (see refs 5, 6, 7 and the ‘Methods’ section for details). The latter method describes polaronic states derived from the potential energy surface of the neutral charge state (equation (11) in the ‘Methods’ section) that may be induced on ionization. In our MBPT approach, the resultant SF yields only the lowest energies of these polaronic states with combination of single vibrations belonging to different dynamic distortions of the geometry. The broadening of these polaronic states due to change of the geometry on ionization involving multiple vibration excitations is accounted for by the HR method.
Figure 1 clearly demonstrates that the HR approach of vibrationassisted ionization energies does not account for the experimental PES when the overall lineshape and the broadening of the QPs are considered (see Fig. 1a). Instead, the manybody SFs convolved by HR broadening reproduce remarkably well the overall lineshape of the experimental PES and the broadening of QPs. In particular, the agreement between the experiment and theory is excellent for the adamantane structure in a wide range of photoionization energies: all broad features are correctly described as composed of two local peaks that physically represent coherent packets of electron–vibration states (Fig. 1b). For the other two diamondoids, the dynamical electron–vibration interaction significantly improves the calculated lineshapes compared with the HR method. We emphasize that the broadening is well described not just for the ionization of the highest occupied molecular orbitals but for the deeper states too.
Analysis of the QP states
In order to understand the calculated PES, we analyse the electronic structure and vibrational modes of the structures we have considered. The lowest unoccupied molecular orbital (LUMO) and the high energy states are very diffuse Rydberg states^{18}. As a consequence, their coupling to the vibrational modes is small, and their SFs (see ‘Methods’ section) exhibit an almost perfect QP line shape. The calculated QP shifts (see ‘Methods’ section) ΔE_{n} for n=LUMO,LUMO+1,…. due to electron–vibration coupling are in the region of 0.05–0.01 eV and the renormalization factors (see ‘Methods’ section) Z_{n} are greater than 0.95. Here, LUMO+1 refers to the index of the state above the LUMO. The situation changes significantly in the case of the highest occupied molecular orbital (HOMO) and lower energy occupied states (HOMO1, HOMO2 and so on.), which are the only ones contributing to the PES. These occupied states are localized on the atoms constituting the diamond cages and are strongly coupled to the atomic vibrations. This coupling induces Z_{n}<0.7 for all these states. Values for Z_{n} far from one clearly point to a potential breakdown of the electron QP picture (in the limit of Z_{n}=0, purely electronic states do not exist). In simple terms, this is confirmed and visualized by the presence of multiple peaks with wellobservable intensities appearing in the manybody SFs and in the calculated PES. These states rule out any description in terms of single and welldefined electronic energy states. We note that the breakdown of electron QP states has also been found in other carbon–hydrogen systems, polymers^{7,8}, and strong renormalization of QP levels led to a decrease of around 7% in the calculated direct gap of bulk diamond^{24}.
SF of adamantane and the Jahn–Teller effect
Now we analyse the nature of the calculated SFs represented by the coloured curves in Fig. 1a. We start our analysis with adamantane. The HOMO of adamantane is mostly localized on the C–C sp^{3} orbitals forming a triple degenerate t_{2} state within T_{d} symmetry. Its SF shows two peaks (see Fig. 2a): the main peak is at around 9.25 eV and a second satellite peak at around 10.0 eV. This contributes to around 2 eV broadening of the HOMO, which well reproduces the broadening observed in the experiment (see Fig. 1). The main peak might be associated with the electron QP level that would result in a 0.24 eV shift for the HOMO (for example, the shift between the green dotted line and the maximum peak in the green curve at around 9.5 eV in Fig. 1a). This is a large correction and, more importantly, it corresponds to a QP charge Z_{n}=0.64. This clearly points to the presence of strong dynamical corrections that break the QP picture. Indeed the smaller the QP charge, the larger the participation of the particle in states where the electronic component is minor compared with the vibration excitations. In this case, the state loses a large fraction of its electronic character. Next, we demonstrate the strength of the MBPT approach in the analysis of the complex photoemission spectrum.
The main peak of the HOMO SF comes from the coupling to 36 different vibrational modes in the region of 124–162 meV corresponding mostly to C–C stretch modes. The largest contribution is due to a T_{2} vibrational mode at 159.8 meV (see Supplementary Note 1, Supplementary Table 1 and Supplementary Movies 4–6). Most of the other coupled vibration modes are degenerate and an A_{1} fully symmetry mode is only weakly coupled. The degenerate vibrational modes coupled to the HOMO of the neutral adamantane move the atoms out of the high symmetry geometry and include the 159.8 meV T_{2} mode, which dynamically distorts the high T_{d} symmetry geometry to a C_{3v} symmetry as demonstrated in Fig. 3a. The DFT calculations of the ionized adamantane in the quasistatic limit result in C_{3v} distortion that was partially discussed previously^{22,25}: the T_{2} HOMO state is a Jahn–Teller (JT) system on ionization leaving a hole in the triple degenerate state that may be described as a t_{2}⊗T_{2} vibronic state. We find that the 159.8 meV T_{2} vibrational mode that mostly leads to formation of coherent packets of electrons and breaks the QP picture is the same that drives the JT distortion of the ionized adamantane. This finding indicates that the vibronic states found by MBPT induce the JT effect. The link between these effects can be explained by the fact that the linear JT coupling (see Fig. 2 of ref. 26 and references therein) corresponds to the absolute square of the electron–vibration coupling (g in Equation 4 in the ‘Methods’ section) which is strong for the t_{2} HOMO in the neutral adamantane according to our calculations. This strong electron–phonon coupling is manifested in the PES via the calculated SF that contains the amplitude of the transition between the ionized and neutral systems in the MBPT approach (see Lehmann representation of the SF in the ‘Methods’ section). This shows that our MBPT approach indicates the JT nature of the ionized systems. This is a particularly important finding as this can be extended to the degenerate states lying below the HOMO level.
By following this argument other important conclusions can be drawn in the interpretation of the calculated SF and the experimental PES. The second peak of the HOMO SF corresponds to a satellite that originates from the coupling to 43 different degenerate vibrational modes with energy of 78–158 meV. These states correspond to the twist and bending modes of C atoms. The largest contribution belongs to the 78.2meV T_{2} twist mode (see Supplementary Note 1, Supplementary Table 1 and Supplementary Movies 1–3). These twist modes do not appear in bulk diamond but only in the quasi zerodimensional diamond cages and lead to a dynamical symmetry distortion that is peculiar for these systems. Analogue to the main HOMO SF peak, this satellite HOMO SF peak can be associated with the motion of atoms in the ionized system that distorts the T_{d} symmetry due to JT effect. We refer to it as anomalous JT distortion by following Patrick and Giustino^{25}. Remarkably, our MBPT approach is able to identify the origin of the satellite HOMO peak in PES and implies a link to the JT effect. We further note that these twist modes contribute to the second local maximum in the first broad feature of the PES of adamantane at around 10 eV (for example, Figs 1a and 2a).
Comparison of adamantane and urotropine
At this point, it is intriguing to compare the t_{2} HOMO states of adamantane and urotropine that share the same T_{d} symmetry but show distinct shape of PES for HOMO (see Fig. 1b). We compare the HOMO SFs for adamantane and urotropine in Fig. 3. The HOMO in urotropine is strongly localized on the four N atoms. It couples to 39 (20) different vibrational modes in the energy region of 56 (56) meV to 93 (129) meV for the main (satellite) peak (see Supplementary Note 1 and Supplementary Table 3). This results in about 1.5 eV broadening of HOMO in urotropine that is about 0.5 eV smaller than that in adamantane. Furthermore, the main and the second peaks originate from a coupling with a fully symmetric A_{1} vibrational mode of 128.6 meV (see Supplementary Movie 10). In the second peak, the contribution of a T_{2} vibrational mode of 82.7 meV may imply a JT distortion (see Supplementary Movies 7–9). In the main peak, the coupling to many degenerate vibrational modes appears but only with a minor weight. We find by quasistatic DFT calculations on the ionized urotropine that the JT distortion is minor and the atoms move with a smaller amplitude upon ionization than those in adamantane. In other words, the JT effect is smaller in urotropine than in adamantane. The proposed link between MBPT SF of the neutral system and the JT effect of the ionized system is in line with this finding: a stronger JT effect results in a wider electron–vibrationrelated broadening in PES. This feature is well captured by our MBPT approach.
Analysis of deep QP states of adamantane
We continue the analysis of PES for adamantane in Fig. 1. As we mentioned earlier, the second local maximum at around 10 eV can be explained by the satellite peak of the HOMO. However, it is evident from the dotted curve in Fig. 1a that lowenergy satellite peaks of the closely lying HOMO1 and HOMO2 states also contribute to that. The HOMO1 t_{1} and HOMO2 e states are degenerate and also subject to the JT distortion upon ionization. Indeed, the lowenergy satellite peak, the main peak and the highenergy satellite peak originate mostly from the coupling to different degenerate vibrational modes (see Fig. 2b,c, respectively) that dynamically distort the T_{d} symmetry in both cases. The main peak and the highenergy satellite peak of HOMO1 and HOMO2 states contribute to the shape of the second broad feature in the PES of adamantane. Finally, similar conclusion can be drawn for the third and fourth broad features in PES. The third broad feature corresponds to the HOMO3 t_{1} and HOMO4 t_{2} states that are triple degenerate and subject to JT distortion again. Their SFs are shown in Fig. 2d,e, respectively. As the broadening of these states due to electron–vibration coupling is very large (above 2.5 eV), their SFs strongly overlap despite the relatively large QP energy gap of 0.4 eV (for example, orange dotted lines and the corresponding orange curves under the third broad feature of black curve in Fig. 1a). Particularly, the four peaks that are visible in the SF of HOMO4 clearly demonstrate the breakdown of the electron QP picture. We found that more than 100 different vibrational modes within an energy range of 37–365 meV couple to this electronic state and contribute to the corresponding peaks in the SF. We note that the dynamic distortion of the 147.2 meV mode in the HOMO3 SF couples to the HOMO4 state whereas the dynamic distortion of the 173.1 meV mode in the HOMO4 SF couples to the HOMO3 state. The final lineshape of the calculated PES is very asymmetric and it is well represented by the calculated SFs convolved by HR method. A very similar process is responsible for the asymmetry of the fourth broad feature originating from the HOMO5 and HOMO6 states and the broad features in urotropine composed from HOMO1 to HOMO4 states.
Signature of pseudo Jahn–Teller effect in diamantane
Next, we analyse the PES of diamantane with D_{3d} symmetry. The calculated SFs of diamantane HOMO and the lower energy states are very broad and create an almost featureless PES, in good agreement with the experiment (Fig. 1b). The HOMO and the HOMO1 states, the fully symmetric nondegenerate a_{1g} and the double degenerate e_{g} states are localized mainly on the C atoms. The HOMO2, HOMO3 and HOMO4 states are characterized by e_{u}, a_{1u} and e_{u} symmetry, respectively.
First, we focus our attention on the HOMO and HOMO1 and their interaction. Although a_{1g} and e_{g} states are principally distinct in nature, their SFs look very similar (see the green and yellow curves with a maximum at around 9.0 eV in Fig. 1a). By recalling our proposal for a link between the strength of JT coupling and the width of broadening in PES based on the analysis of the HOMO in adamantane and urotropine, this might be surprising since the nondegenerate a_{1g} state is stable against JT distortion whereas the double degenerate e_{g} state is not.
We anticipate that this phenomenon is a manifestation of the socalled pseudoJahn–Teller effect^{27}. We explain this feature in conjunction with the HOMO of adamantane and their relation to the valence band edge of bulk diamond. The valence band edge of diamond at the Γpoint is a tripledegenerate t_{2g} under O_{h} space group neglecting the spin–orbit interaction. This t_{2g} state is built up from the linear combination of sp^{3} hybrid valence orbitals of carbon atoms. Adamantane, as a single cage of diamond, forms very similar tripledegenerate HOMO orbital with a correspondence of O_{h}:t_{2g}→T_{d}:t_{2}. Diamantane with two diamond cages forms a lower symmetry, so O_{h}:t_{2g}→D_{3d}:a_{1g}+e_{g}; the original tripledegenerate state of diamond ‘HOMO’ orbital splits to a nondegenerate and a double degenerate state. Nevertheless, this splitting does not originate from the chemical nature of the bonds but from the low symmetry of ions, thus these states have hidden connection, and they may be considered as pseudodegenerate states. This is the reason why the SFs of adamantane's HOMO t_{2} and diamantane's HOMO a_{1g} and HOMO1 e_{g} orbitals have very similar SF lineshapes. The 159.8 meV T_{2} mode, the most responsible for the JT distortion of adamantane HOMO (main peak in SF), appears as 162.7 meV A_{1g} mode for HOMO (see Supplementary Movie 13) and 159.0 meV E_{g} mode for HOMO1 in diamantane (see Supplementary Movies 11,12) where similar correspondence can be derived between these vibrational modes (see Fig. 4) as for their electronic states. Particularly, the zcomponent of the tripledegenerate T_{2} vibrational mode of adamantane is mimicked by the fully symmetric A_{1g} vibration mode in diamantane. These A_{1g} and E_{g} vibrational modes distort the diamond cages of diamantane similarly to the corresponding components of the T_{2} vibrational mode of adamantane (Fig. 4b). Thus, A_{1g} vibrationrelated motion of atoms represents a pseudoJT distortion of the diamond cages in diamantane upon ionization. To summarize, the vibrational modes that lead to formation of coherent packets of electrons and vibrational modes and break the QP picture are the same that drive the pseudoJT distortion. The hidden connection between the electronic states can be analysed by the corresponding MBPT SFs.
We discuss further the PES of diamantane. The second peak in the SF of HOMO and HOMO1 states of diamantane shows a similar anomalous JT distortion to that of the HOMO of adamantane. Going further with the group theory analysis, the HOMO2 and HOMO3 e_{u} and a_{1u} states have a correspondence to the adamantane's HOMO1 t_{1} state, while the HOMO4 e_{u} state has a relation to the adamantane's HOMO2 e state. However, as the symmetry of the two e_{u} states are the same in diamantane, these electronic states can mix the character of the ascendant t_{1} and e states of adamantane. This also results in a much larger number of vibrational modes that couple these two e_{u} electronic states compared with the coupling of the t_{1} and e states in adamantane (for example, Supplementary Table 1 versus Supplementary Table 2). The computed PES shows an almost featureless shape at around 10.3 eV for diamantane, in contrast to the corresponding spectrum at around 11.0 eV for adamantane (see Fig. 1b). Thus, the difference in the broadening and the lineshape of the two diamondoids could be well explained by the analysis of their orbitals, coupling of states via vibrations, and the proposed JT effects upon ionization.
Discussion
We note that the fine structure of the experimental PES consisting of sharp features requires further discussion. Our HR spectrum on the diamondoids suggests (see red curves in Supplementary Fig. 1) that the fine structure could be related to the ionizationinduced changes in the geometry. However, the accurate calculation on the strength of this contribution requires to consider the dynamical and geometryinduced effects on the same footing. This is equivalent to extend the present MBPT approach to include multiple vibrational excitations in the form of a vertex correction. Our MBPT approach has to be extended to capture multiple vibrational excitations, and we anticipate that vertex corrections can account for this. Inspired by the success of the present combined HR+MBPT approaches, we are actively pursuing the development of this more comprehensive theory.
In conclusion, we demonstrated on small nanodiamonds that the electron–vibration coupling results in the breakdown of the electron QP picture for their occupied states even at zero temperature. This has serious consequences on the features of their photoemission spectra, which cannot be predicted by semiclassical vibration broadening of electron states. We found indications in our MBPT approach for the fingerprint of different JT distortions. Our results imply that understanding of all the experimental features in the photoexcitation or photoionization of small nanoparticles needs a detailed investigation of electron–vibration coupling. We showed that our fully ab initio MBPT approach is capable of studying realistic systems and analyse the role of vibrations in their photoionization processes. This makes possible to design structures where the vibrations are manipulated to achieve the desired optoelectronic properties, which is of immediate importance in the field of superconductors, photovoltaic materials, colour centres in nanodiamonds^{4} and related materials^{28} for nanometrology.
Methods
Groundstate calculations
The groundstate geometry and electronic structure of the diamondoids were computed by plane wave supercell KSDFT calculations as implemented in the Quantum Espresso (QE) software package^{29}. We used a simple cubic simulation box and a diamondoid–diamondoid separation of about 1 nm to avoid the spurious interaction between the periodic images. For diamantane, we applied a hexagonal box to have a simulation box commensurable with its point group symmetry. The core electrons were taken into account by using normconserving Troullier–Martins pseudopotentials^{30}. We took the standard Troullier–Martins pseudopotentials for each atom from the QE database except for nitrogen where we applied a relatively soft pseudopotential. We found that a kinetic energy cutoff of 45 Ry for plane wave expansion was sufficient to converge the band gap of the selected diamondoids. We applied ab initio LDA within KSDFT to calculate the total energy and the KS spectrum^{31,32}. The geometry of the diamondoids was optimized by minimizing the Hellmann–Feynmann forces below the threshold of 0.001 Ry per Bohr. In the geometry optimization procedure, we applied 80 Ry kinetic energy cutoff. We aligned single particle energies to the vacuum level by using the Martyna–Tuckerman method^{33} as implemented in QE. The vibrational frequencies were computed by density functional perturbation theory^{34}. The calculations were performed with a strong threshold of 10^{−16} Ry to achieve the selfconsistent total energy in order to obtain accurate vibrational modes.
The implemented HR method to calculate vibration broadening
The rotations of single diamondoids and their collisions with other cages cause a broadening of about 20 meV (ref. 14) that does not explain the two orders magnitude larger broadening in the experimental PES. This is due to the relatively strong electron–vibration coupling where high energy vibration states with n>0 quantum number contribute to the PES. The vibrationassisted ionization spectrum can be calculated by the HR method^{35} within the Franck–Condon approximation that is explained briefly as follows. The key equation is the SF of electron–phonon coupling^{36}
where the sum is over all vibration modes λ with frequencies ω_{λ}, and S_{λ} is the partial HR factor for the mode λ. S_{λ} basically is the strength of the electron–vibration coupling of vibration λ. This can be defined as
where
m_{α} is the mass of atom α, i=x,y,z, R_{{I,N};αi} is the equilibrium position in the ionized (I) and neutral (N) state and Δr_{λ;αi} is normalized vector that describes the displacement of the atom α along the direction i in the vibration mode λ. On ionization of the diamondoids, the optimized geometry changes from neutral to the ionized state within our Born–Oppenheimer approximation calculated by the chosen DFT. The vibration modes of the neutral diamondoids are calculated by the density functional perturbation theory method. The total HR factor S is obtained by . Generally, if S<<1 then the spectrum is very sharp and mostly localized at the position of the QP energy. If S>10, then the spectrum is very broad, featureless and can be well described with a symmetrical Gaussian function. We found that the typical value for diamondoids, S∼3, leads to a more complicated structure. The spectrum consists of a few sharp features lying on a broad background and the shape of the spectrum is nonsymmetric. The S∼3 implies that three vibration quanta should contribute to the spectrum. To create a simplified curve for broadening, we replaced the structured HR SF with a continuous envelope function. In the Supplementary Methods and the corresponding Supplementary Fig. 1, we give a more detailed description about this methodology and the results on the selected diamondoids.
The dynamical approach to the electron–vibration problem
Our methodology has been derived in detail in refs 6, 7. Here, we only briefly summarize the basic assumptions and the key equations. Since we have finite objects within the supercell formalism, we use the k=0 in the Brillouin zone and thus the momentum transfer q is also set to zero.
Using finite temperature MBPT, one can derive the self energy of an electron due to its interaction with vibrational modes. We consider the lowestorder selfenergy terms: Fanterm () and DWterm () (refs 6, 7). Both depend on the temperature (T) through the boson occupation number of the vibration states (B(ω_{λ})):
Here, n and are the KS electron states with KS energies ɛ_{n} and , respectively. f_{n} is the Fermi function of electrons. Since the diamondoids have large gaps, f_{n} is 1(0) for occupied (unoccupied) states, respectively. is the electron–vibration matrix element between states n and due to the vibrational mode λ and energy ω_{λ}. This is a linear combination of weighted by the amount they contribute to each vibrational mode, where is the change in the selfconsistent potential due to the displacement R_{α,S} of atom s along the cartesian direction α. We compute the firstorder derivatives of the KS potential using density functional perturbation theory^{34}. The secondorder derivatives appearing in equation (5) () can be turned into products of firstorder derivatives by using translational invariance. In the summations over we used 200 states and checked convergence by using 300 states for selected diamondoids. In the summations over λ, we did not include the first six modes corresponding to translations and rotations of the diamondoids.
The temperaturedependent Greenfunction due to electron–vibration interaction can be written as
By Taylor expanding the Fan term around the unperturbed energies, we can also define perturbative corrections to the electron QP states:
where the renormalization factor Z_{n}(T) reads
The QP shift ΔE_{n}(T) due to electron–vibration interaction may be simply defined as ΔE_{n}(T)=E_{n}(T)−ɛ_{n}. We note that the PES for diamondoids was measured at room temperature. For adamantane, we checked that bosonic occupation of vibration states indeed do not change the results going from zero kelvin up to room temperature. Since N–C, C–C and C–H vibrational modes have much higher energies than the room temperature energy of 26 meV, only the groundstate vibration states have nonzero occupations, and thus the calculated properties do not show measurable temperature dependence in the region of zero kelvin and room temperature. Therefore, we omit the temperature dependence in the QP shift ΔE_{n}≡ΔE_{n}(T) and the renormalization factor Z_{n}≡Z_{n}(T).
We can also compute the SF, which is defined as
where G_{n}(ω) is taken from equation (6) by omitting the temperature. These SFs are plotted for a given n KS state in Fig. 2 for adamantane from which the PES was derived as shown in Fig. 1b. We note here that equation (9) does not include transition matrix element effects and thus our method of computing PES corresponds to a constant, energyindependent transition matrix element approximation.
For the analysis of the contribution of the vibrations to the corresponding SFs for a given KS state, we use the Lehmann representation,
where E_{I} is the energy of the true eigenstate () of the system and η is a small infinitesimal number. is the exact ground state and c_{n} is the electron annihilation operator. Here, we again omit for simplicity the temperature dependence. By definition, E_{I} are the real poles of G_{n}(ω).
In ref. 7, it was shown that the states are mixed packets of electrons and vibrations. Moreover, their internal structure was found by showing that the electron–vibration problem can be fully rewritten as the solution of an effective Hamiltonian. The solution of this problem allows to introduce an explicit expression for the interacting states :
is the purely electronic state obtained by creating an electron in the nth KS level. is the corresponding probability to find the electron–vibration state along . , instead, is the probability to find the fully interacting state in a mixed electronic and vibrational λ state (see refs 7, 37). These coefficients can be found by diagonalizing the electron–vibration Hamiltonian on the basis of equation (11). This tool was applied to analyse the contribution of vibrations λ to the given peaks in the SFs, for instance, as depicted in Fig. 2 for adamantane.
From the Lehmann representation, it follows that the Greenfunction represents the dynamical evolution of the charged state . This situation is quite similar to the physics described in the Jahn–Teller effect. The difference is that, in the present case, the atoms are allowed to move only within the harmonic approximation. Nevertheless, as done in ref. 26, the analysis of the terms can be used to deduce the most intense phonon modes (and consequently, atomic displacement directions) that contribute to the formation of the coupled electron–vibration states.
The complex structure of the state, then, induces the wealth of structures that are crucial to explain the PES and, at the same time, provides a sound and clear indication of the most intense modes that contribute to the physics of the Jahn–Teller effect.
Additional information
How to cite this article: Gali, A. et al. Electron–vibration coupling induced renormalization in the photoemission spectrum of diamondoids. Nat. Commun. 7:11327 doi: 10.1038/ncomms11327 (2016).
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Acknowledgements
A.G. acknowledges the support from the Lendület program of the Hungarian Academy of Sciences, the PRACE DECI6 DIASIC project and the PRACE DECI7 DIAVIB project (FP7 RI283493) for the resources CINECA in Italy and HUYGENS in Netherlands. The technical assistance of Andrew Emerson from CINECA and Dr Jörg Hertzer from High Performance Computing Center, Germany is gratefully acknowledged. A.G. and M.V. also acknowledge the support from the NIIF Supercomputer Center Grant No. 1090. A.M. acknowledges financial support by the Futuro in Ricerca grant No. RBFR12SW0J of the Italian Ministry of Education, University and Research MIUR, the European Union project MaX Materials design at the eXascale H2020EINFRA20151, Grant agreement No. 676598 and Nanoscience Foundries and Fine Analysis  Europe H2020INFRAIA20142015, Grant agreement No. 654360. This work was also supported by U.S. DOE, Office of Science under Contract No. DEAC0206CH11357 (M.V.). This research used resources of the National Energy Research Scientific Computing Center, a DOE Office of Science User Facility supported by the Office of Science of the U.S. Department of Energy under Contract No. DEAC0205CH11231.
Author information
Affiliations
Institute for Solid State Physics and Optics, Wigner Research Centre for Physics, Hungarian Academy of Sciences, PO Box 49, H1525 Budapest, Hungary
 Adam Gali
 , Tamás Demján
 & Gergő Thiering
Department of Atomic Physics, Budapest University of Technology and Economics, Budafoki út 8, H1111 Budapest, Hungary
 Adam Gali
 & Gergő Thiering
Institute of Physics, Loránd Eötvös University, Pázmány Péter sétány 1/A, H1117 Budapest, Hungary
 Tamás Demján
Materials Science Division, Argonne National Laboratory, Lemont, Illinois 60439, USA
 Márton Vörös
Institute for Molecular Engineering, University of Chicago, Chicago, Illinois 60637, USA
 Márton Vörös
AixMarseille Université, CNRS, PIIM UMR 7345, 13397 Marseille, France
 Elena Cannuccia
Institute for Material Science (ISM) of the National Research Council (CNR), Via Salaria Km 29.3, CP 10, 00016 Monterotondo Stazione, Italy
 Andrea Marini
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Contributions
A.G. proposed the idea and the strategy for the calculation on the effect of electron–vibration coupling in the QP states, and wrote the paper. T.D., G.T. and M.V. carried out the calculations whereas E.C. and A.M. developed the manybody perturbation theory and implemented into the applied scientific code. A.G. and G.T. implemented the Huang–Rhys method. All the authors discussed the results and commented on the manuscript.
Competing interests
The authors declare no competing financial interests.
Corresponding author
Correspondence to Adam Gali.
Supplementary information
PDF files
 1.
Supplementary Information
Supplementary Figure 1, Supplementary Tables 13, Supplementary Note 1 and Supplementary Methods
Videos
 1.
Supplementary Movie 1
The video shows the vibration mode T_{2(x)} at 78.2 meV for adamantane. The carbon and hydrogen atoms are depicted by brown and white balls, respectively.
 2.
Supplementary Movie 2
The video shows the vibration mode T_{2(y)} at 78.2 meV for adamantane. The carbon and hydrogen atoms are depicted by brown and white balls, respectively.
 3.
Supplementary Movie 3
The video shows the vibration mode T_{2(z)} at 78.2 meV for adamantane. The carbon and hydrogen atoms are depicted by brown and white balls, respectively.
 4.
Supplementary Movie 4
The video shows the vibration mode T_{2(x)} at 159.8 meV for adamantane. The carbon and hydrogen atoms are depicted by brown and white balls, respectively.
 5.
Supplementary Movie 5
The video shows the vibration mode T_{2(y)} at 159.8 meV for adamantane. The carbon and hydrogen atoms are depicted by brown and white balls, respectively.
 6.
Supplementary Movie 6
The video shows the vibration mode T_{2(z)} at 159.8 meV for adamantane. The carbon and hydrogen atoms are depicted by brown and white balls, respectively.
 7.
Supplementary Movie 7
The video shows the vibration mode T_{2(x)} at 82.7 meV for urotropine. The carbon, nitrogen and hydrogen atoms are depicted by brown, blue and white balls, respectively.
 8.
Supplementary Movie 8
The video shows the vibration mode T_{2(y)} at 82.7 meV for urotropine. The carbon, nitrogen and hydrogen atoms are depicted by brown, blue and white balls, respectively.
 9.
Supplementary Movie 9
The video shows the vibration mode T_{2(z)} at 82.7 meV for urotropine. The carbon, nitrogen and hydrogen atoms are depicted by brown, blue and white balls, respectively.
 10.
Supplementary Movie 10
The video shows the vibration mode A_{1} at 128.6 meV for urotropine. The carbon, nitrogen and hydrogen atoms are depicted by brown, blue and white balls, respectively.
 11.
Supplementary Movie 11
The video shows the vibration mode E_{g(x)} at 159.0 meV for diamantane. The carbon and hydrogen atoms are depicted by brown and white balls, respectively.
 12.
Supplementary Movie 12
The video shows the vibration mode E_{g(y)} at 159.0 meV for diamantane. The carbon and hydrogen atoms are depicted by brown and white balls, respectively.
 13.
Supplementary Movie 13
The video shows the vibration mode A_{1g} at 162.7 meV for diamantane. The carbon and hydrogen atoms are depicted by brown and white balls, respectively.
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