Ab Initio Simulations of Core Level Spectra Towards an Atomistic Understanding of the Dye-Sensitized Solar Cell

Ab initio simulations of core level spectra Towards an atomistic understanding of the dye-sensitized solar cell

Ida Josefsson c Ida Josefsson, Stockholm 2013

Distributor: Department of Physics, Stockholm University List of Papers

This thesis is based on the following papers, referred to in the text by their Roman numerals.

PAPER I: Ab Initio Calculations of X-ray Spectra: Atomic Multiplet and Molecular Orbital Effects in a Multiconﬁgurational SCF Approach to the L-Edge Spec- tra of Transition Metal Complexes I. Josefsson, K. Kunnus, S. Schreck, A. Föhlisch, F. de Groot, Ph. Wernet, and M. Odelius, The Journal of Physical Chemistry Letters 2012, 3 (23), 3565-3570. DOI: 10.1021/jz301479j

PAPER II: Collective Hydrogen-Bond Dynamics Dictates the Electronic Structure of − Aqueous I3 I. Josefsson, S. K. Eriksson, N. Ottosson, G. Öhrwall, H. Siegbahn, A. Hagfeldt, H. Rensmo, O. Björneholm, and M. Odelius, Submitted to PCCP.

− − PAPER III: Energy Levels of I /I3 in Solution from Photoelectron Spectroscopy S. K. Eriksson, I. Josefsson, N. Ottosson, G. Öhrwall, O. Björneholm, A. Hagfeldt, M. Odelius, and H. Rensmo, In Manuscript.

Reprints were made with permission from the publishers. Contents

List of Papers iii

Abbreviations vi

1 Introduction 7

2 Computational framework 10 2.1 Born-Oppenheimer approximation ...... 10 2.2 Quantum chemical methods ...... 10 2.2.1 The independent particle model and self-consistent ﬁeld theory . . . . . 11 2.2.2 Electron correlation ...... 12 2.2.3 Multiconﬁgurational theory – the active space ...... 13 2.2.4 Perturbation theory ...... 15 2.2.5 Relativistic effects ...... 15 2.3 Solvation models ...... 16 2.3.1 Molecular dynamics ...... 16 2.3.2 Polarizable continuum ...... 18

3 Core-level spectroscopy 19 3.1 Photoionization ...... 19 3.1.1 Chemical shifts ...... 20 3.1.2 The sudden approximation and shake-up processes ...... 20 3.2 X-ray absorption and emission ...... 21 3.3 Peak intensities ...... 22 3.3.1 Linewidths and shapes of x-ray spectra ...... 23 3.3.2 Photoemission intensities ...... 23 3.3.3 RIXS intensities ...... 23

4 Transition metal complexes 25 2+ 4.1 [Ni(H2O)6] ...... 25

− − 5 I /I3 in water, ethanol, and acetonitrile solutions 28 5.1 Solvated I− ...... 28 − 5.2 Solvated I3 ...... 29 Acknowledgements xxxii

References xxxiii Abbreviations

AO Atomic orbital BO Born-Oppenheimer CASPT2 Second-order perturbation theory with CASSCF reference function CASSCF Complete active space self-consistent field CI Configuration interaction DSC Dye-sensitized solar cell HF Hartree-Fock HOMO Highest occupied molecular orbital LMCT Ligand-to-metal charge transfer LUMO Lowest unoccupied molecular orbital MD Molecular dynamics MLCT Metal-to-ligand charge transfer MO Molecular orbital PCM Polarizable continuum model PES Photoelectron spectroscopy QC Quantum chemistry RASSCF Restricted active space self-consistent field RDF Radial distribution function RIXS Resonant inelastic x-ray scattering SCF Self-consistent field SIBES Solvent-induced binding energy shift UV/Vis Ultraviolet-visible spectroscopy XAS X-ray absorption spectroscopy XPS X-ray photoelectron spectroscopy 1. Introduction

The world energy consumption is growing rapidly. Fossil fuels still provide 80 percent of the energy consumed in the world [1]. Both for environmental reasons and because the resources are finite, understanding and developing renewable energy sources is however desirable. The sunlight reaching the Earth’s surface every hour would be sufficient to cover the world’s entire need for energy over the next year [2], but solar energy still accounts only for a slight fraction of the world energy sources [1]. The first important property of a solar cell converting light into electrical energy is that it is able to absorb sunlight. Next, charges – electrons and holes – must be separated, and transported through the cell and an outer circuit, where the current can be used for external work. The amount of energy is determined by the voltage over the cell. Finally, the photogenerated charges should be collected in order to enter a new photocycle. The silicon device yet dominates the solar cell market, but photovoltaics based on molecular materials is a promising competitor for low cost production. One such is the dye-sensitized solar cell (DSC) [3], shown schematically in Figure 1.1. In the DSC, an organic or transition metal-based dye absorbs light. The dye is attached to a nanoporous wide-bandgap semiconductor surface, often TiO2, that does not absorb in the visible spectrum. An electrolyte, traditionally − − the I /I3 redox couple dissolved in an organic solvent, mediates electrons between the elec- trodes. Other material combinations have also shown great potential for use in the DSC; recent

− I3

I−

Figure 1.1: An illustration of the components of the DSC: a dye-sensitized nanoporous semiconductor surface surrounded by an electrolyte. The arrows show the electron current when light is converted to electricity. developments include replacing the dye with an inorganic semiconductor and the electrolyte with a solid molecular hole conductor [4–7]. The standard dye-electrolyte cell described here is however the model commercially available.

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srdcdback reduced is sNHE vs V (1.1) − /I − 3 − metal systems is the strong spin-orbit coupling, and particularly for transition metals also the multiconﬁgurational character of the system. An important part of the computational work is a correct treatment of these effects and accurate modeling of excited states, including charge transfer effects.

Outline

The computational methods and models used for the calculations in Paper I-III are described in Chapter 2 in this thesis. Chapter 3 gives an overview of the relevant core-level spectroscopic techniques. Many of the ﬁgures illustrating the concepts in Chapter 2 and 3 are based on the actual models and/or results in the work described in Paper I-III, although the main part of the results is summarized in Chapter 4 and 5. Based primarily on Paper I, the topic of Chapter 4 is x-ray absorption and resonant inelastic scattering spectroscopy of transition metals, while − − Chapter 5 gives a summary of photoelectron spectroscopy studies of I and I3 in solution (Paper II and III).

9 2. Computational framework

The typical picture of a molecule is a composite of charged particles: nuclei and electrons. The fundamental interaction, determining the chemistry and properties of an atom or a molecule in its environment, is the Coulomb interaction between these particles. Every system can be described by equations – solving the differential equation describing a chemical system provides information about all its properties and processes.

2.1 Born-Oppenheimer approximation

Since it is not possible to separate the degrees of freedom for the internal motion of more than two interacting particles, the differential equations for all chemical systems larger than the hydrogen atom must be solved numerically. However, physical properties can often be used for an approximate separation of variables. In the Born-Oppenheimer (BO) approximation [9], the motion of the heavy nuclei and the light electrons are assumed to occur on different timescales: In the electron’s perspective, the nuclei appear ﬁxed. Due to their large mass, atoms and molecules can usually be well described with classical dynamics, whereas the wave-like character of the electrons has to be treated with quantum mechanics. Consequently, we rely on quantum chemical (QC) methods for calculating electronic spectra. In order to capture the effect of the strong intermolecular interactions in solution, a large number of individual solvent molecules needs to be taken into account. In practice, it is not possible to describe the solvent molecular motion with quantum mechanics, but molecular dynamics (MD) can be used to simulate the solution dynamics.

2.2 Quantum chemical methods

The central equation in quantum mechanics is the Schrödinger equation [10]: ∂Ψ(r,t) H(r,t)Ψ(r,t) = i , (2.1) ∂t where the Hamiltonian H is the sum of the kinetic and potential energy operators, with the time dependence of the Hamiltonian contained in the potential energy operator. The solution to the Schrödinger equation gives the wavefunction Ψ, from which all information about the system can be extracted. The time and space variables of the wavefunction can be separated and for a time-independent potential, the total energy of the system is given by the time-independent Schrödinger equation, an ordinary differential equation:

H(r)Ψ(r) = E(r)Ψ(r). (2.2)

10 If the coupling between the nuclear and electronic motion is neglected (BO-approximation), the total wavefunction Ψ separates into an electronic and a nuclear part. The electronic wavefunction depends parametrically on the nuclear coordinates R, and the corresponding eigenvalues ε(R) create a potential energy surface on which the nuclei move. The nuclear equation can then be solved on the electronic surface, which yields a set of rotational and vibrational levels.

2.2.1 The independent particle model and self-consistent field theory The potential energy operator corresponding to Coulomb repulsion between the electrons in the electronic Hamiltonian is not separable. The independent particle approximation decouples the complex dynamics of a many-electron system to single-particle problems, through the as- sumption that an individual electron moves independently of the dynamics of the others. The corresponding part of the Hamiltonian can hence be replaced by the interaction of the electrons with the average field in which they move. In the independent particle model, a molecule can be described with a set of one-electron wavefunctions. The one-electron Hamiltonian contains the kinetic energy of the electron and the potential energy of the electron in the field of the nuclei. With each independent electron is associated a spatial function ϕ – an orbital – and a corresponding energy eigenvalue, obtained by solving the Schrödinger equation with this Hamiltonian. Not only the spatial function, but also the spin, describes the electron. However, an N- electron wavefunction cannot simply be expressed as a product one-electron space and spin functions (spin orbitals) χ – it also has to be antisymmetric in order to obey the Pauli exclusion principle [11]. In the Hartree-Fock method [12; 13], the approximate wavefunction is formed by a Slater determinant [14] with the N occupied spin orbitals – for a molecule, the molecular orbitals (MOs) – arranged in columns and the electron coordinates in rows:

χ1(1) χ2(1) ... χN(1)

1 χ1(2) χ2(2) ... χN(2) = √ . (2.3) Ψ . . .. . N . . . .

χ1(N) χ2(N) ... χN(N)

The determinant ensures that the antisymmetry criterion is fulﬁlled. The wavefunction expressed as a single determinant as in Equation 2.3, can be reduced to a set of one-electron differential equations1, resembling single particle Schrödinger equations (the Hartree-Fock equations):

0 0 Fiχi = εiχi , (2.4) where Fi is the Fock operator, containing four terms: the kinetic and electron-nuclei potential energy contributions, which depend only on the coordinate of electron i, and two terms that sum over all electron positions. These two-electron operators contain the electrostatic repulsion between the electrons (the Coulomb operator Ji j) and a nonclassical term (the exchange operator Ki j). The last term results from the Pauli principle and eliminates the probability of two electrons

1 Since the determinant remains the same under an unitary transformation, we can choose χi to be an 0 orthonormal set of molecular orbitals χi .

11 with the same spin to occupy the same position in space. The solutions to the HF equations are 0 molecular orbitals χi with the corresponding orbital energies εi. In the ground state N-electron wavefunction, N orbitals are occupied successively in increasing energy, beginning at the lowest corresponding orbital energy. The highest occupied orbital (HOMO) and the lowest unoccupied (LUMO) are particularly important when studying photo- chemistry, since the lowest possible excitation from the ground state typically is an electronic transition from the HOMO to the LUMO. The MOs are complicated mathematical functions, but can be expanded in a set of basis functions. Often, a set of functions φα localized at the nuclei is chosen, and each MO is then expressed as a linear combination of these known “atomic orbitals” (AO)

M χi = ∑ cαiφα , (2.5) α=1 where M is the number of basis functions. The unknown MO coefﬁcients cαi must be calculated 1 iteratively, by minimizing the total energy of the wavefunction. The resulting eigenfunctions χi which are solutions to the HF equations are called self-consistent ﬁeld (SCF) orbitals. With N MOs occupied, the M − N empty functions in the basis set are referred to as virtual orbitals.2 From now on, I am going to omit the spin coordinate and refer to MOs as spatial orbitals, containing at most two electrons with opposite spins.

2.2.2 Electron correlation The two assumptions described in Section 2.2.1 – that each electron interacts only with the average field created by the other electrons and that the wavefunction can be written as a single Slater determinant – introduces an error in the wavefunction and the total energy. The difference between the exact energy of the system and the HF energy is usually called the correlation energy. The electron correlation can be separated into two categories: static and dynamic. For systems where the wavefunction is not dominated by a single Slater determinant, the (long-range) static correlation is important. This is often the case in transition-metal complexes: because of the mixing of electronic configurations, HF fails to describe the ground state. The dynamic (“instantaneous”) contribution to the correlation energy is short-range and re- flects the decreased probability of finding electrons near each other due to the Coulomb and Pauli repulsion. Even though HF theory accounts for the correlation between electrons with the same spin (Pauli repulsion), it neglects the correlated motion between electrons with opposite spins, since the Coulomb repulsion from the other electrons is only seen as an average field. The HF single determinant is an approximation of the wavefunction Ψ, but in fact any N- electron wavefunction can be expanded exactly in an infinite number of Slater determinants. A better approximation of Ψ can thus be formed by adding determinants with different electron

1The variational theorem states that the exact ground state energy is always less than or equal to the expectation value of the Hamiltonian calculated for an approximate wavefunction. 2The HF wavefunction depends only on the energies of the occupied orbitals, and the virtual orbitals have no direct physical meaning.

12 configurations, that is, Slater determinants with electrons occupying other orbitals than the reference HF determinant. The exact wavefunction would be obtained as a linear combination of Slater determinants, where all possible ways of arranging electrons are included in a complete AO basis set: ∞ Ψ = a0ΦHF + ∑aSΦS + ∑aDΦD + ... = ∑ akΦk, (2.6) S D k=0 where the determinants have been grouped into configurations describing single (S), double (D), etc. excitations. ΦHF is the HF wavefunction in Equation 2.3. In the configuration interaction method (CI) [15], a set of orthonormal MOs – the orbital coefficients cαi in Equation 2.5 – is first obtained from a HF calculation and kept fixed. For a given set of MOs, the weight of each determinant is calculated variationally, i.e. by finding the coefficients that minimize the energy. In practice a complete CI is not attainable, but a finite basis set is used. Full CI (even for a finite basis set) is computationally very expensive, and instead the series is truncated to contain determinants up to a given excitation level (single, double, etc excitations). The coefficients that minimize the total energy are the eigenvectors of the Hamiltonian in the same basis of determinants.

2.2.3 Multiconfigurational theory – the active space An alternative way of treating the multiconfigurational character is by optimizing not only the coefficients ak for the determinants, but also the MO coefficients cαi. The complete active space self-consistent field (CASSCF) method [16] selects the configurations included in the wavefunction by a partitioning of the MOs into an active and an inactive space. The inactive orbitals are all doubly occupied. In the active space, all orbital permutations consistent with the number of electrons and spin multiplicity are allowed, i.e. a full CI is performed, and for all configurations, the orbital coefficients are optimized. Since excited configurations are included in the CASSCF wavefunction, the calculation gives, in addition to the ground state, all the excited states that can arise from these. When calculating transitions between electronic states, the choice of active space can hence be used as a direct tool to control that the excitations of interest are covered. The main challenge with the CASSCF method is that the computational cost grows rapidly with the number of MOs included. To keep the calculation manageable, the active space can be further divided into three subspaces, with certain limitations in the occupation numbers, or equivalently: excitations. This method is referred to as the restricted active space SCF (RASSCF) method [17]. The QC calculations described in Paper I-III are multiconfigurational calculations, performed with the Molcas-7 software [18]. 2+ The [Ni(H2O)6] complex in Figure 2.1 serves as an illustration of the RASSCF method. The first subspace, RAS1 is chosen to comprise the Ni 2p core orbitals. The RAS1 orbitals would be doubly occupied in the HF, but in this particular RASSCF calculation, one hole is allowed. RAS2 consists of the orbitals of nominal Ni 3d character with no restrictions on the occupation. The remaining occupied orbitals are left inactive: the orbital coefficients are optimized in the CASSCF procedure, but the orbitals are not involved in the excitations. The total number of electrons in RAS1 and RAS2 is fixed and we can therefore separate the possible excitations into

13 ∗ 2b2 H2O ∗ Valence excitation 4a1 eg Ni 3d RAS2 t2g 1b 1 Core excitation H2O 3a1 1b2 H2O 2a1 Ni 3p Ni 3s

H2O 1a1 Ni 2p RAS1 Ni 2s

Ni 1s

2+ Figure 2.1: Molecular orbital diagram of Ni (H2O)6. The active space in the RASSCF calculation comprises the RAS1 and RAS2 subspaces with 14 electrons in 3+5 MOs. The Ni 2p core orbitals in RAS1 can contain at most one hole, while the occupation in the Ni 3d orbitals in RAS2 is unre- stricted. With the possible electron conﬁgurations included in the RASSCF, the energy of valence excited states (transitions indicated by red arrow) and states with a 2p core hole (blue arrow) can be accessed (Paper I).

two types: (1) configurations with one hole in RAS1, and an “extra” electron in RAS2 and (2) configurations with RAS1 fully occupied. The first case corresponds to core-excitations 2p→3d (with a single core hole), and the second case includes all valence excitations corresponding to pure d-d transitions. The dominant configuration for the ground state is the one shown in Figure 2.1, with eight electrons populating the “3d” MOs in a high-spin fashion. At this point it is however worthwhile to recall the two parts in the RASSCF procedure: First, that the CI coefficents are optimized for the specific state, and therefore excited configurations also give a small contribution to the ground state wavefunction. Second, the MO coefficents are optimized for the selected states, which implies that the nominal 3d orbitals are to some extent mixed with ligand orbitals, i.e. hybridized. In the calculations in this work, the energies are calculated using a single set of orbitals, optimized for the energy average of all included states of a given spatial and spin symmetry (state-averaging). The example in Figure 2.1 does not allow for excitations from the occupied orbitals on the water ligands to the metal center: ligand-to-metal charge transfer (LMCT). Neither can excitations from the metal center to the unoccupied ligand orbitals – metal-to-ligand charge transfer (MLCT) – take place. To model MLCT, we can however introduce a third subspace, RAS3, of (in the HF) unoccupied ligand orbitals, containing a limited number of electrons. Similarly, occupied ligand orbitals can be incorporated in the active space to take LMCT into account.

14 2.2.4 Perturbation theory

The added ﬂexibility in the wavefunction in the CAS(RAS)SCF approach mainly recovers the static correlation. The remaining dynamical correlation can be included either perturbatively or with subsequent multireference CI (MRCI) calculations [19; 20]. We chose to work with many-body perturbation theory, with the general idea that the solution only differs slightly from the simpler, already solved problem, constituting the “reference” and can be added as a perturbation. The Hamiltonian of the N-electron wavefunction is then partitioned into a reference and a perturbation Hamiltonian [21]. In second order perturbation theory, the perturbation Hamil- tonian is a two-electron operator. All combinations where two electrons from occupied (in the reference wavefunction) orbitals are excited to virtual orbitals are taken into account in the correction to the energy. The second order perturbation approach CASPT2(/RASPT2) uses a CASSCF(/RASSCF) reference wavefunction. In the CASPT2 calculations of multiple states in the present work, multistate CASPT2 [22] has been used, where the included states are allowed to mix.

2.2.5 Relativistic effects

The Schrödinger equation (Equation 2.1) does not take the consequences of the finite speed of light, affecting both orbital sizes and shapes, into account. Also, magnetic interactions due to the electron spin, spin–orbit coupling, is a relativistic effect. Relativistic corrections affect the chemistry of light elements less, but for heavier elements, the effects are important. The relativistic wave equation for a free electron – the Dirac equation [23] – is a four- dimensional equation: in addition to two spin degrees of freedom, the Hamiltonian contains two components arising from the electron–positron coupling. The Hamiltonian of the N-electron system is assumed to be as sum of such one-electron terms (and potential energy operators). Solving the full four-component equation is however computationally very demanding; in a Douglas- Kroll-Hess transformation [24; 25], the wavefunction is reduced to two components. The relativistic calculations in Paper I-III have been calculated according to the Douglas-Kroll-Hess scheme implemented in Molcas, partitioning the relativistic effects into a spin-free (scalar) and a spin–orbit part: In the first step, a set of multiconfigurational and correlated states (RASSCF or RASPT2) is computed, via a scalar Hamiltonian. The spin–orbit Hamiltonian (approximated by a one-electron effective Hamiltonian, within the mean-field model [26]) for this set of wavefunctions is then calculated in a subsequent step [27].

In Figure 2.2, the energies of the spin-free and spin–orbit states of neutral I3 with a single − 4d core hole are shown, relative to ground-state I3 . At the 4d level, the orbitals are atomic like and localized on the respective nuclei. The states can be distinguished by the site on which the core hole is localized: center or terminal. The origin of the different levels is discussed in further detail in Chapter 5. Calculating the spin–orbit part of the Douglas-Kroll Hamiltonian, with the spin-free states as a basis – in other words: letting the spin and orbital momenta couple – leads to the splitting of the 4d level of almost 1.6 eV.

15 CASPT2 CASPT2+SO 51.83 Ω = 5/2 51.87 Ω = 3/2 51.88 Ω = 1/2 51.88 Ω = 3/2 52.46 (2) Λ = 2 51.89 Ω = 5/2 51.91 Ω = 1/2 52.51 (1) Λ = 0 52.51 (2) Λ = 1 52.51 (2) Λ = 1 52.52 (2) Λ = 2 53.42 Ω = 3/2 52.55 (1) Λ = 0 53.45 Ω = 1/2 53.46 Ω = 3/2 53.47 Ω = 1/2 53.59 Ω = 5/2 53.87 Ω = 3/2 54.04 Ω = 1/2 54.23 (2) Λ = 2 54.58 (2) Λ = 1 54.73 (1) Λ = 0

55.26 Ω = 3/2 55.59 Ω = 1/2

Figure 2.2: Energies of the 4d core hole states of isolated I3, relative to the ground state energy − of the I3 anion (in eV). The energies to the left are calculated in a spin-free CASPT2 framework, including scalar relativistic effects. Since the set of 4d orbitals on each atom is associated with ﬁve ml quantum numbers, there are in total 3·5=15 possible electron conﬁgurations with one 4d core hole, the corresponding states characterized by Λ. Lines in blue represent states where the electron has been removed from a 4d orbital on the central iodine atom (the degeneracy is given in parentheses), while red denote states with a core hole on either of the two terminal atoms. The spin–orbit states in the right column are obtained from interaction of the spin-free states. Diagram from Paper III.

2.3 Solvation models

So far, we have dealt only with the idealized, static, case with molecular geometries optimized to an energy minimum and without any interaction with surrounding molecules. In reality, the problem contains both dynamics and environmental effects. The experiments in Paper II and III were done in solution, and in Chapter 3 we shall see the solute–solvent interactions described in more detail. The solvent effects can essentially be introduced in the calculations in two ways: by implicit or explicit modeling.

2.3.1 Molecular dynamics Just like the QC calculations described in Section 2.2, MD simulations rely on the BO approximation, but in contrast to calculating the electronic structure as a function of the nuclear coordinates, the electrons are accounted for as a single parametric potential energy surface. No electrons are hence explicitly included in the calculations, and N now refers to the number of atoms (or sometimes molecular fragments) in the system. As its name suggests, MD does not

16 just give a static description of the system, but models the time-evolution. However, the atoms are assumed to obey classical dynamics, and by numerical integration of Newton’s equations of motion d F = m x˙ = mx¨ , (2.7) i dt i i information about how all particles move over a period of time can be obtained. After calculating the resulting force on each atom from its neighbors, the particles are allowed to move under the constant force for a short timestep. The forces are then recalculated for the new positions. A classical MD simulation requires a force field describing, first, the ion–solvent and solvent– solvent (intermolecular) interactions and, second, the intramolecular interactions. Often, the Lennard-Jones potential [28] describes the pairwise van der Waals interactions between atoms and a Coulomb potential the electrostatic contribution to the intermolecular interactions, each atom represented by a point charge. Intramolecular interactions – bending and stretching of the molecule – can be modeled as harmonic potentials. In addition, suitable initial and boundary conditions have to be chosen. In the preparation of Paper I-III, ions in solution were simulated with MD and the average solvation structure was investigated. A number of configurations of the studied ion was also sampled during its motion in the solution. Part of the sampling was done with the purpose of studying the pure configurational effects; then the solute geometries representing the distribution was extracted from the MD simulations and treated with QC. For inclusion of solvent effects, a shell of the closest solvent neighbors were also included in the QC calculation. Furthermore, in Paper II, the real-time evolution of the bond lenghts in the triiodide ion was traced. The classical MD simulations were performed under constant volume and temperature, using periodic boundary conditions, with the simulation box replicated in all directions to simulate bulk.

Ab initio molecular dynamics The predefined potentials used in classical MD (usually based on empirical data or independent QC calculations), are not able to describe changes in the electronic structure and hence no bond breaking and formation. In ab initio MD, the electronic degrees of freedom are actu- ally taken into account, as the potential is obtained from a QC calculation in every timestep. Instead of a suitably parametetrized force field, a method for solving the Schrödinger equation hence has to be selected. Two ab initio MD methods are Born-Oppenheimer (BOMD) and Car-Parrinello (CPMD). In BOMD the wavefunction is optimized to the ground state in every timestep [29]. CPMD instead includes the electrons as ficticious particles moving at a different timescale than the nuclei, avoiding computationally expensive wavefunction optimization iterations as the wavefunction remains close to the one optimized for the initial nuclear geometry [30]. A very short timestep is however required.

Radial distribution functions MD trajectories can be analyzed in terms of radial distribution functions (RDFs). The RDF g(r) gives the probability of ﬁnding two different atom types separated by the distance r, relative to a uniform distribution. Figure 2.3 shows ion–water RDFs for I− in aqueous solution. Since

17 I − O I − H g(r)

2 3 4 5 6 Distance / Å Figure 2.3: I–water radial distribution functions (RDFs) for I− in aqueous solution. Thick lines corresponds to the I–O RDF and thin lines to I–H RDF. The first iodine-hydrogen maximum at 2.6 Å interatomic separation results from hydrogen bonding. the RDF maxima correspond to the distances from the ion at which water oxygen and hydrogen spend the most time during the simulation, they are directly related to the hydration shells around the ions. As expected for an anion, the I–H RDF in Figure 5.4 shows that the water hydrogen is coordinating the iodide ion in aqueous solution, with a well-defined RDF maximum at 2.6 Å – i.e. at a typical hydrogen bond length – and the oxygen peak about 1 Å outside this maximum. A less ordered second hydration shell is formed outside the first solvation sphere. We shall return to the triiodide ion in solution in Chapter 5.

2.3.2 Polarizable continuum Rather than considering explicit solvent molecules, continuum models take the configurational averaging implicitly into account through macroscopic properties of the solvent, while the solute is treated quantum mechanically. In the Polarizable continuum model (PCM) [31], the solute is placed in a cavity in a uniform polarizable medium with a dielectric constant ε characterizing the solvent. Point charges on the cavity surface represent the reaction field created due to the polarization of the solvent in the presence of the solute. This reaction field in turn perturbs the solute itself. By adding the reaction field perturbation in the Hamiltonian, the Schrödinger equation can be solved self-consistently, thus including the effect of the environment.

18 3. Core-level spectroscopy

The core electrons of a molecule do not participate in the chemical bonding; unlike valence orbitals, they are localized on the atomic nuclei and have well separated binding energies associated with them, typically in the x-ray region of the electromagnetic spectrum. In contrast, the molecular bonds are – in a molecular orbital description – formed by valence electrons in orbitals delocalized over the entire molecule. The valence binding energies lie closer than the core levels and often in the range of visible or ultraviolet light. Since each chemical element has its characteristic pattern of wavelengths at which it absorbs light, x-ray spectroscopy can be used to gain element-specific information of the material. This section gives a brief description of characterization techniques employing x-ray radiation. The techniques can be classified according to what is detected: in the first case, the material is ionized and the ejected electrons detected (photoelectron spectroscopy) and in the second case, the absorption and possibly subsequent emission of x-rays is measured (x-ray absorption and resonant inelastic x-ray scattering spectroscopy). [32–37]

3.1 Photoionization

The basis of photoelectron spectroscopy (PES) is the photoelectric effect [38; 39]. If the energy hν of photons illuminating a surface is sufﬁciently high – at least equal to the binding energy BE of a speciﬁc electron – an electron can be released from the material. According to the photoelectric law, the photoelectron is emitted with kinetic energy

KE = hν − BE. (3.1)

In x-ray photoelectron spectroscopy (XPS), the amount of electrons escaping the sample after interaction with x-rays is measured as a function of their kinetic energy. The resulting spectrum is represented as a graph of the intensity against the binding energy. XPS is thus used to probe the occupied levels. If the electronic transition from the initial state |0i (with N electrons) to the ﬁnal state | f i (with N −1 electrons + a non-interacting photoelectron) takes place on a timescale much shorter than the typical timescale for molecular vibrations, the molecular geometry can be assumed not to change during the transition. However, the sudden decrease in screening of the nuclear charge upon ionization “immediately” causes relaxation of the outer orbitals. In such a vertical transition, the binding energy, expressed as the energy difference between the ﬁnal and initial states BE = E(N−1) − E(N), (3.2) includes electronic, but not nuclear, relaxation.

19 The experimental photoelectron spectra in Paper II and III were measured by collaborators, using synchrotron radiation at MAX-lab in Lund and BESSY at the Helmholtz-Zentrum Berlin. The liquid samples were injected into the experimental chamber as a micro jet [40–42].

3.1.1 Chemical shifts Even though core electrons do not participate directly in the chemical bonding, the core binding energies are affected by the chemical environment. These chemical shifts, in the order of a few eV, add site-speciﬁc information to the spectra of chemical compounds: Two chemically inequivalent atoms (of the same element) have different core binding energies, due to the differences in nuclear screening depending on the valence charge distribution on the surrounding atoms. In addition, the spectra of solutions provide information of the solute–solvent interaction. Ionization of the solute changes both the solvent polarization and the solvent-induced polarization of the solute, which leads to a shift of the binding energy – solvent-induced binding energy shift (SIBES) – with respect to photoionization in the gas phase. When the photoelectron leaves an anion, the negative ion charge decreases, thus weakening the electrostatic interaction between solute and solvent. In contrast, the positive charge of a cation increases upon photoemission. Figure 3.1 shows that this results in a positive SIBES for an anion and negative for a cation.

gas solvated gas solvated LiI(aq) I Li2+

62 60 58 56 54 52 50

Gas (theo.) I4d Intensity / Arb. units Li1s I− Li+

77 75 73 52 50 48 46 Binding energy (eV)

Figure 3.1: The solvent-induced binding energy shifts of the Li+ and I− peaks in the photoelectron spectra (left ﬁgure) have opposite signs. The scheme to the right illustrates that this is due to that the electrostatic interaction either vanishes (anion) or increases (cation) upon electron removal. The black arrows in the right ﬁgure represent the binding energies, and the SIBES corresponds to the change in binding energy when going from gas phase to solution. (Spectra from Paper III.)

3.1.2 The sudden approximation and shake-up processes For rapid photoionization processes, the use of the sudden approximation [43] is justiﬁed. The electronic relaxation is then neglected during the ionization process itself: the abrupt change

20 ∗ in the effective potential leaves the system in the same state. This state |Ψ iN, is simply what remains of the N-electron wavefunction after pulling out an electron effectively away from the electrostatic well. It is hence not an eigenstate |ki f of the new Hamiltonian, but can be expressed as a linear combination of the new, electronically relaxed, eigenstates:

∗ |Ψ iN = ∑ck|ki f , (3.3) k where the (real) coefﬁcients ck are given by

∗ ck = f hk|Ψ iN. (3.4) Among the possible eigenstates, states with an unbound electron are found, with the correspond- (N−1) ing energy eigenvalues Ek . The sudden change in electrostatic potential may give rise to shake-up satellites in the spectrum, as the departing core electron interacts with the valence. In this case, the resulting ﬁnal state, which is a proper eigenstate |ki f , can be considered a simultaneous core ionization and valence excitation. The kinetic energy of the photoelectron is thus slightly (a few eV) reduced in the shake-up process.

3.2 X-ray absorption and emission

In x-ray absorption spectroscopy (XAS) the sample is irradiated with x-rays and excited reso- nantly from the initial state |ii to the state | f i with a core electron occupying previously empty valence orbitals. Just as the core-electron binding energies can be attributed to specific atomic sites in the system (Section 3.1), so can core-excitation energies in the XAS process. Conse- quently, measurements of the x-ray absorption intensity as a function of the incident photon energy map the uncoccupied valence states onto a particular atom in the system. The short-lived core-excited state can decay either through emission of a photon or an electron. Resonant inelastic x-ray scattering spectroscopy (RIXS), is applied on the first decay type; the incident energy is scanned across an absorption edge and the intensity of the subse- quently emitted energies is measured over a certain energy range. The RIXS process is described schematically in Figure 3.2. From the law of energy conservation, the emitted photon is seen to have energy ω = Ω − ω f 0, (3.5) where Ω is the energy of the incident photon and ω f 0 the energy loss: the difference in energy between the final and initial states. Decay of the core-excited state back into the ground state gives rise to an elastically scattered peak, where the emitted photon has the same energy as the absorbed photon. There are however other possible decay channels of the core hole, in which the core hole is filled and the system is left in a valence excited state. This is observed as a fluorescence line at an energy a few eV lower than the incident energy. The energy loss corresponds precisely to the valence excitation energy. The resulting two-dimensional RIXS spectrum can hence be used to probe the unoccupied levels with chemical specificity, as a function of the incident energy.

21 Total energy

Em ω Ω

Ef E0

Figure 3.2: The RIXS scattering process. By absorption of a photon with energy Ω, the molecule is excited from the initial state |0i to a metastable intermediate state |mi with a core hole. The system decays to the ﬁnal state | f i under emission of a photon with energy ω. The dashed arrow represents the elastic transition with Ω = ω, and the solid decay to a valence excited ﬁnal state. The energy left in the system (loss) is given by Ω − ω. Adapted from Glatzel et al. [36].

3.3 Peak intensities

The intensity of a peak in a spectrum is directly related to the probability for photon absorption or emission. The most important type of interaction between electromagnetic radiation (such as x-rays) and an atom or molecule is via electric dipole interaction, where the oscillating electric ﬁeld of the radiation perturbs the Hamiltonian due to the interaction with the charge distribution in the system. Within the dipole approximation, the probability that linearly polarized light induces the electronic transition |ii → | f i depends on the transition (dipole) moment between the initial and ﬁnal states:

Mi f = h f |µ|ii, (3.6) where µ is the electric dipole moment operator. Given that Mi f is nonzero, absorption of a photon with energy ωi f can occur if its energy matches the difference between the initial and ﬁnal state energies (Ei and E f ) as expressed in Fermi’s Golden Rule [44]:

2 w fi ∝ |Mi f | δ(E f − Ei − ωi f ), (3.7) where w fi is the transition probability and the delta function takes care of the energy conservation. The RIXS process is more involved than XPS and XAS and addressed in Section 3.3.3.

It is important to note that not only the amplitude of Mi f , but also its direction (the polarization direction) relative to the electric ﬁeld vector of the incident light, determines the absorption probability: absorption is maximal if the vectors are parallel and zero if they are perpendicular to each other. In a kinetic viewpoint, the probability of absorption or scattering is usually given 2 in terms of a cross section, proportional to Mi f .

22 3.3.1 Linewidths and shapes of x-ray spectra One important factor limiting resolution of x-ray spectra is the intrinsic lifetime: due to the time- energy uncertainty relation, the final state energy is only known up to the accuracy determined by the lifetime of the final core-excited state. The lifetime broadening leads to a Lorentzian lineshape. In addition, configurational broadening and experimental resolution (in the energy of the x-ray beam and the analyzer resolution) give rise to a Gaussian distribution of the energies. The configurational broadening can be understood as small chemical shifts caused by geometry fluctuations. Vibronic coupling and fine structure may also give a small Gaussian contribution to the spectrum. The total peak typically has a Voigt profile, namely a convolution of the different broadening mechanisms of Gaussian and Lorentzian character.

3.3.2 Photoemission intensities A fast XPS process, induced by high energy photons, can be considered a sudden annihilation of an electron from the initial state. The initial state wavefunction with an unbound electron in Equation 3.3 can then be expressed as an annihilation operator aq acting on the photoelectron ∗ (the qth electron) in the initial state: |Ψ iN = aq|ΨiN. From the square of the coefﬁcients in Equation 3.4 we obtain the relative XPS intensities Pk within the sudden approximation: 2 Pk ∝ |NhaqΨ|ki f | . (3.8)

Pk thus gives the probability for transitions from the ground state of the N-electron system to the eigenstates |ki f for the core-ionized (N − 1)-electron system – including ﬁnal states with collective core and valence excitations. In the theoretical XPS spectra in the present work, we have however only calculated the binding energies (not the intensities), and added a broadening according to section 3.3.1.

3.3.3 RIXS intensities Since RIXS is a second order process, where the molecule absorbs a photon with energy Ω and emits a photon with energy ω, the first order perturbation term in Equation 3.6 does not provide a sufficient description. Rather than separable absorption and emission processes, the process should be considered a single-step scattering event. The correlation is treated by the Kramers- Heisenberg formula [45], which gives an expression for the scattering amplitude Ff (Ω), containing a sum over all intermediate (core-excited) states. If the intermediate states lie close in energy, the decay channels may interfere, and the interference effects are taken into account in the square modulus of the scattering amplitude: 2 2 Ω − ω − iΓ F (Ω) = ω ω D0†D i0 i , (3.9) f ∑ i f i0 fi i0 2 2 i (Ω − ωi0) + Γi where ωi f and ωi0 are the intermediate-final and intermediate-initial state energy differences 0† (Em − E f and E f − E0 in the scheme in Figure 3.2). D fi and Di0 correspond to the probabili- ties for the transitions and are defined as the projection of the electronic dipole moment µ of

23 the molecule onto the electric field vectors of the incident and emitted light respectively. The remaining complex Lorenzian function adds a broadening of the line due to the finite lifetime Γi of the core-excited state. In the calculated RIXS spectra in Paper I, summarized in Chapter 4, we have however neglected interference and the polarization dependence in D fi and Di0. The total RIXS intensity is obtained by summation over all possible final states, and depends on the energies of both the incident and emitted photons:

2 (ω−Ω+ω f 0) Ω 2 Γ f 1 − 2 . I( , ) F · · √ e γ (3.10) Ω ω ∝ ∑ f 2 2 ω f π((ω − Ω + ω f 0) + Γ f ) πγ

The intrinsic width in the energy loss direction of the spectrum is determined by the ﬁnal state lifetime Γ f in the Lorentzian in the expression above. Experimental and conﬁgurational broadening sets the value of the Gaussian broadening parameter γ.

24 4. Transition metal complexes

Transition metals, with their partially ﬁlled d (or f) valence orbitals, often form coordination complexes that absorb in the visible region and are used as the active site in many energy- related applications. XA and RIXS spectroscopy (Section 3.2) provide rich information about the electronic valence in the presence of a core hole. Calculations that reproduce – and hence can serve as an appropriate basis for interpretation of – the experimental transition metal spectra must handle multiplet effects and chemical interactions properly. Multiplets arise in the spectra due to the coupling between the spin and orbital angular momenta of the core hole and the partly ﬁlled d orbitals. Excitations in the valence are mainly of either of the types referred to in Section 2.2.3: charge transfer (LMCT or MLCT), involving transitions from/to the ligands to/from the metal center, or d-d transitions within the d orbitals on the metal center. Paper I presents ab initio1 2p XAS and RIXS calculations, based on a RASSCF wavefunction, of hydrated Ni2+. Direct comparison of the calculated XA spectra with experiment shows that the approach is highly reliable for 2p spectroscopy of 3d complexes.

2+ 4.1 [Ni(H2O)6]

2+ 8 The Ni (H2O)6 complex has a high-spin d ground state electron conﬁguration and is octa- hedrally coordinated by the water ligands. The XA spectra in Figure 4.1 were calculated with the RAS partitioning described in Section 2.2.3 (Figure 2.1) and spin-free relativistic effects

EXP RASPT2 RASSCF XA intensity

850 855 860 865 870 875 Excitation energy [eV]

2+ 5 9 Figure 4.1: RASSCF and RASPT2 calculated XA spectra of Ni (H2O)6 including all [(2p) ,(3d) ] core-excited conﬁgurations, in comparison with the experimental spectrum of NiCl2(aq).

1Ab initio calculations are based entirely on ﬁrst principles, in contrast to methods that introduce empirical or ﬁtting parameters.

25 treated by a scalar Douglas-Kroll Hamiltonian combined with a relativistic all-electron (ANO- RCC) VTZP basis set [46; 47]. The spin–orbit coupling was calculated between all the singlet and triplet states resulting from this active space (allowing all core excitations leading to a [(2p)5,(3d)9] electron conﬁguration). The large multiplet splitting of the 2p x-ray absorption edge (2p → 3d) is due to the strong spin–orbit coupling of the 2p5 conﬁguration, i.e. the core hole. The method reproduces the features in each of the edges and the dominating core-level spin–orbit splitting in the 2p XA spectrum agrees well with experiment. The additional multiplets within the respective edge arise due to core–valence (2p3d) electron–electron interactions. In order to compensate for limitations in the RASSCF wavefunction, the spectrum (green line) is shifted by -3.70 eV for comparison with experiment. A large part of the ad hoc correction is due to dynamical correlation: The RASPT2 energies (red line) are shifted by the smaller value -1.85 eV.

In the low-energy (L3) peak, final core-excited states with the total core hole angular mo- 3 1 mentum 2 dominate, while states with 2p angular momentum 2 give rise to the (L2) peak above 870 eV. Upon closer examination of each edge, we find that the XA resonance at the low-binding energy side has mainly triplet character. In other words, final states with parallel 2p core hole and 3d electron spins are stabilized with respect to singlet states (opposite spins), which are found in the peak at higher binding energy. We can analyze the valence further, by studying the states resulting from fluorescent decay of the core hole. Equation 3.5 is illustrated schematically in Figure 4.2: the energy difference between the x-rays absorbed and emitted in the RIXS process corresponds to the energy of the final, possibly valence excited state relative to the ground state. The calculations give explicit

850 855 860 865 870 875

5 ∗ a) Valence 2b2 H2O ∗ excitation 4a1 0 Energy loss [eV] eg Energy Ni 3d RAS2 loss b) XAS t2g

1b1 H O 3a 2 1 XA Intensity 1b2 1 850 855 860 865 870 875 H2O 2a1 c) 0 Ni 3p 15 Ni 3s -1 X-ray H2O 1a1 10 -2 absorption Ni 2p RAS1 -3 5 Ni 2s Energy loss [eV] -4

Ni 1s -5 Logarithmic RIXS Intensity 0 -6 850 855 860 865 870 875 Excitation energy [eV]

Figure 4.2: Each core-excitation has its particular set of decay channels from the intermediate state in the RIXS process to ﬁnal valence excited states. (a) RIXS map, with the intensity as a function of the x-ray absorption energy and the associated energy loss, and (b) the corresponding XA spectrum from RASPT2 calculation including [(2p)6,(3d)8] and [(2p)5,(3d)9] conﬁgurations. (c) Charge-transfer states are included by increasing the number of orbitals in the active space.

26 access to each electronic state; guided by the extracted information, we can both assign the lines in the XAS spectrum, and unearth the electronic character of every final valence state resulting from RIXS at a specific absorbed photon energy. The RASPT2 spectra in panel a and b in Figure 4.2 are obtained from the same calculation as the previous XA spectra, namely without including ligand orbitals in the active space. The possible electron permutations in the 3d orbitals 6 2 5 3 4 4 correspond to three different configurations: (t2g) (eg) , (t2g) (eg) , and (t2g) (eg) . Analysis of the L3 edge RIXS shows that the XA resonance at 853 eV (triplet) – apart from the peak at zero energy loss, corresponding to resonant elastic decay from the core-excited inter- 3 mediate back to the ground state ( A2g) – decays with high intensity to two peaks at 0.9 eV and 3 2.9 eV loss. The peaks originate from decay to the T2g valence excited state (essentially de- 5 3 3 scribed by the (t2g) (eg) configuration) and to T1g, respectively. These two states are formally 3 3 3 3 equivalent to the final states resulting from the optical transitions A2g → T2g and A2g → T1g in UV/Vis spectroscopy [48]. Since RIXS is a second-order process and the spin multiplicites in the valence mix in the intermediate core-excited state, final valence states that are optically spin-forbidden may also be reached; the XA peak at 866 eV (singlet character) decays with high probability to singlet final states. In the RIXS spectrum in panel c, the active space has been extended, and the contribution from charge-transfer excitations arise at an energy loss above 10 eV. Here, two occupied water orbitals have been added to RAS2, thus enabling transfer of electrons to the metal centered 3d orbitals (LMCT). A third subspace (RAS3), consisting of three unoccupied ligand orbitals, is also created. Since one electron is now allowed in RAS3, MLCT as single excitations to the unoccupied ligand orbitals is taken into account. Information about photochemical processes, such as those in the DSC, is found in the time evolution of the nuclear geometry and valence electronic structure. With this method, also XA and RIXS spectra of distorted geometries and transient electronic states can be modeled, and used in the analysis of time-resolved experiments – probing changes in the electronic structure with atomic site selectivity on the femtosecond timescale.

27 − − 5. I /I3 in water, ethanol, and acetonitrile solutions

− − The I /I3 redox couple has been used as the hole conducting medium in the DSC for a long time, but the redox chemistry is still only partially understood. Information about the fundamental solvation phenomena and the energies involved is useful for the understanding of the redox − − mechanisms. Paper II and III describe the solvation of I and I3 in different solvents, where we have used core-level PES to study the electronic structure. Multiconﬁgurational QC calculations combined with MD simulations give an insight in the microscopic details, supported by and supporting the analysis of liquid jet experiments. We observe a large dependece on the local − − solvent structure in the solvation energies of I and I3 . The short-range solvent interactions are − also important for the I3 molecular structure, even leading to symmetry breaking in aqueous solution.

5.1 Solvated I−

The magnitude of the binding energy shift in solution varies with the solvent: Through the series water → ethanol → acetonitrile, the I4d photoelectron spectra in Figure 5.1 show a decreased SIBES. The trend is connected with the type of interaction – and hence amount of stabilization – in the solution; water and ethanol form hydrogen bonds to the ion, while acetonitrile is a polar solvent without hydrogen bonds. Strong hydrogen bonding leads to a large solvation energy, and consequently large core-level SIBES to lower binding energy for the anion (see Section 3.1.1). The solvent structure is important for the stabilization of the ion: The I4d SIBES of I− dissolved in ethanol (forming hydrogen-bonded chains or clusters) is weaker than in aqueous solution. Static continuum models, such as PCM, are therefore not able to capture the trend; a microscopic solvation description is needed. The SIBES computed using PCM in Table 5.1 is slightly overestimated and essentially the same for the three different solvents. Calculations of clusters with explicit solvent molecules take the short-range solute–solvent interactions such as hydrogen bonding into account and reproduces the relative energy ordering of the shifts. The main challenge with this approach is however to treat clusters sufﬁciently large to describe the solvation in bulk at the high QC level. The experimental SIBES is derived from the difference between the binding energy measured in liquid experiments and gas-phase CASPT2+SO calculated values. The active space in the CASSCF/CASPT2 calculations consisted of the 4d orbitals and the 5s, 5p valence, with the orbitals optimized for the energy average of the 4d orbitals.

28 AcCN EtOH Water Gas (theo.)

SIBES Intensity / arb. units

58 56 54 52 50 48 Binding energy / eV

Figure 5.1: Experimental 4d core level photoelectron spectra of I− in different solvents and the spin-orbit coupled CASPT2 spectrum of the isolated ion. The SIBES is deﬁned as the difference between the gas and solvated peak positions. Figure from Paper III.

Table 5.1: Experimental and calculated solvent-induced I4d electron binding energy shifts (SIBES) in water, acetonitrile, and ethanol. The theoretical values are obtained within the PCM model at the CASPT2+SO level of theory and with CASSCF+SO calculations of cluster conﬁgurations sampled from MD simulations of LiI in solution. Table adapted from Paper III.

SIBES Water Ethanol Acetonitrile Experimental 4.18 3.66 3.39 PCM (CASPT2+SO) 5.33 5.18 5.25 Cluster: 1st shell (CASSCF+SO) 2.80 ± 0.40 1.47 ± 0.37 1.36 ± 0.14 Cluster: 2nd shell (CASSCF+SO) 3.84 ± 0.27

− 5.2 Solvated I3

− In its ground state, I3 is symmetric, with the bond length of the isolated molecular ion calculated to 2.91 Å (CASPT2+SO). Most of the electron density is localized at the terminal sites, which essentially share the net negative charge (-1). Recall now the binding energy diagram in Figure 2.2, where photoelectrons emitted from core orbitals on the central site could be distinguished from those originating from one of the terminal atoms. The reason is the excess of valence charge on the terminal iodine atoms, that results in less strongly bound core electrons on the terminal iodine sites. The 4d core hole on the two equvialent terminal atoms give rise to degenerate states, but with the hole localized on either on them. − What is then the effect of solvation on I3 ? Ethanol and acetonitrile solutions containing − I3 are studied with XPS in Paper III. The local structure of the SIBES not only affects the − magnitude of the SIBES, but also the I3 geometry; Paper II lays a particular focus on the strong coupling between the structural rearrangement of the solvent and the solute dynamics in aqueous − I3 , leading to molecular symmetry breaking. The ﬁgures in this section are found in Paper II. − Other studies (e.g. [49]) show that I3 is linear and symmetric when dissolved in polar solvents, such as acetonitrile, but is distorted in hydrogen-bonding solvents. The experimental ace-

29 tonitrile I4d spectrum can easily be decomposed into terminal and center contributions, consistent with the respective contributions calculated for a symmetric molecular ion (CASSCF+SO), in the middle ﬁgure in panel b. The spectrum from ethanol solution can be deconvoluted in the same manner and is shown under the theoretical spectrum in Figure 5.2b.

MD/CASSCF EXP Total a) b) c) − ∆r I3 I − (g) MD 0.55 Å 3 LiI − I2(g) I3 (aq) MD CASSCF 0.52 Å H2O 0.32 Å

0.29 Å CASSCF I − (g) OPT 0.25 Å 3

0.16 Å AcCN

0.14 Å

Intensity / Arb. units Terminal 0.10 Å EXP Center 0.10 Å EtOH EtOH 0.05 Å 60 58 56 54 52 60 58 56 54 52 60 58 56 54 52 Energy / eV Energy / eV Energy / eV

− Figure 5.2: (a) CASSCF+SO I4d photoelectron spectra of I3 in 10 different conﬁgurations, ordered according to bond length symmetry. (b) Top: Average of the spectra in (a), of the isolated ion (red) and surrounded by a layer of explicit water molecules (violet). Middle: Calculated spectrum of − optimized I3 , showing lines arising from photoemission on the center and terminal atoms separately. − Bottom: Experimental spectrum of I3 dissolved in ethanol, decomposed into terminal and center − contributions. (c) Experimental I3 spectra in water (top), acetonitrile (middle) and ethanol (bottom).

Water’s strong hydrogen bonding ability, however, leads to large bond length ﬂuctuations of − the I3 ion in aqueous solution. Figure 5.3 shows the bond length distribution during a CPMD simulation of LiI3(aq) and includes extremely distorted geometries, with I–I distances well over − the typical covalent bond. The geometry distortions are associated with polarization of the I3 ion: in the observed partial dissociation, the major fraction of the negative charge is localized at the partially detached iodine (with very little change in the center atom charge). Hence, we should expect shifts of the core electron binding energies of a strongly distorted triiodide ion with respect to the gas-phase optimized conﬁguration. The spectra in panel a in Figure 5.2 are − calculated for isolated I3 , with geometries sampled from the MD solution simulation, and show that the degeneracy of the terminal I4d levels is lifted, shifting the peaks in opposite directions with increasing bond-length asymmetry. In Figure 5.4, water–triiodide RDFs are decomposed into separate RDFs for each of the iodine atoms: the center atom and the iodine atoms at the longest and shortest distance from the center iodine in each timestep. The hydrogen RDF for the iodine at the longest separation (which is also the more negative side of the molecule) has a pronounced maximum that coincides

30 4.0

left right long short 3.8

3.6

3.4

3.2

I−I distance / Å 3.0

2.8

2.6 0 10 20 30 40 Time / ps Distribution

Figure 5.3: The time evolution in the I–I bond lengths contains periods of a pronounced asymmetry, highlighted by sampling of the longest and shortest I–I bond. with the ﬁrst maximum of the iodide ion. This signal of hydrogen bonding between iodine and water is absent in the coresponding RDFs for the central atom and the closest iodine. From this we understand that the charge localization is also correlated with the solvent polarization. The geometry distortions, linked with the rearrangement of the water molecules in the hydrogen bond network, can explain the fact that the experimental photoelectron spectrum of aqueous triiodide, shown in panel c in Figure 5.3 (top), is not easily decomposed as in the other solvents.

I − O I − H Iterminal,short Icenter Iterminal,long

I−(aq)

− g(r) I3 (aq)

− I3 (aq)

2 3 4 5 6 Distance / Å

− − Figure 5.4: I (aq) (top) and I3 (aq) (middle+bottom) RDFs. Thick lines corresponds to I-O and thin lines to I-H RDFs. The bottom ﬁgure distinguishes between the iodine atoms with respect to their distance to the central atom (“short” or “long”). Only the iodine the farthest from the center atom (red line) shows a distinct iodine-hydrogen maximum, at close to 3 Å interatomic separation.

− The asymmetry of the I3 ion may favor iodide polymerization in aqueous solution, and hence be important for the stability of the DSC: Water impurities could speed up the aging process, due to polymerization. The coupled solute–solvent dynamics could also inﬂuence the DSC performance through the effect of large geometry distortions on the interactions between − I3 and dye or semiconductor surface.

31 Acknowledgements

Everything described here was done with the support from others. First, my supervisor Michael Odelius: thank you for your genuine help and constructive advice from the very beginning, and Håkan Rensmo for continuous encouragement. This thesis is really a result of working closely together with people doing the real liquid experiments – Susanna Kaufmann Eriksson, I sure − − enjoy our teamwork. That pertains to everybody involved in the I /I3 story; I am grateful for the enlightening discussions and nice collaboration with you in Uppsala (and at new address). Many people have been helpful through different theory and technical discussions. A signiﬁcant part of my time at work is spent staring at a Molcas input or output – in particular, Ulf Wahlgren has been taking the time to explain many a RASSCF-related matter. And, Roland Lindh: Thanks for helping us tame those bizarre PCM calculations. Considering another great experimental collaboration, with you at Helmholtz-Zentrum Berlin: I learned a lot (and still do) from your engaged input to the Ni(II)-project. Finally, to all of you comprising the Chemical Physics Division at Fysikum: I’m glad that you do. References

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