Open access peer-reviewed chapter

# Theoretical Insights into the Topology of Molecular Excitons from Single-Reference Excited States Calculation Methods

By Thibaud Etienne

Submitted: June 12th 2017Reviewed: August 24th 2017Published: December 20th 2017

DOI: 10.5772/intechopen.70688

## Abstract

This chapter gives an introduction to qualitative and quantitative topological analyses of molecular electronic transitions. Among the possibilities for qualitatively describing how the electronic structure of a molecule is reorganized upon light absorption, we chose to detail two of them, namely, the detachment/attachment density matrix analysis and the natural transition orbitals strategy. While these tools are often introduced separately, we decided to formally detail the connection existing between the two paradigms in the case of excited states calculation methods expressing any excited state as a linear combination of singly excited Slater determinants, written based on a single-reference ground state wave function. In this context, we show how the molecular exciton wave function plays a central role in the topological analysis of the electronic transition process.

### Keywords

• excited states
• excitons
• detachment/attachment
• transition matrix and orbitals
• charge transfer

## 1. Introduction

Providing a quantitative insight into light-induced electronic structure reorganization of complex chromophores remains a challenging task that has attracted a substantial attention from theoretical communities in the past few years [1, 2, 3, 4, 5, 6, 7, 8, 9, 10, 11, 12, 13, 14, 15]. Indeed, a potential knowledge related to the ability of a chromophore to undergo a charge transfer caused by photon absorption or emission [16, 17] is of seminal importance for designing novel dyes with highly competitive optoelectronic properties [18, 19, 20, 21]. Most often, such quantitative probing of the charge transfer locality is accompanied by a qualitative study of the rearrangement of the electronic distribution in the molecule, and the aim of this contribution is to demonstrate how in certain cases different topological paradigms are formally connected, with the junction point being the definition of the molecular exciton wave function.

The outcome of the computation of the molecular electronic excited states using a quantum calculation method is, in addition to the transition energy, a series of mathematical objects allowing one to analyze the transition topology. If the reference ground state wave function is, in a given basis (called the canonical basis), written as a Slater determinant, any excited state written based on this ground state wave function is called a single-reference excited state. From this single reference and in a given canonical basis, some methods express excited states as a linear combination of singly excited Slater determinants, which means that the excited state wave function is written as a pondered sum of Slater determinants constructed from the ground state reference, in which one occupied spinorbital (vide infra) is replaced by a virtual one. This type of excited state construction is often referred to as a configuration interaction (CI) solely involving singly excited Slater determinants. In our case, the reference ground state wave function can be a Hartree-Fock or a Kohn-Sham Slater determinant, and the excited states calculation methods we deal with in this paper are called configuration interaction singles (CIS), time-dependent Hartree-Fock (TDHF), random-phase approximation (RPA), Tamm-Dancoff approximation (TDA), or time-dependent density functional theory (TDDFT). For more details about the machinery of these methods, see Refs. [22, 23, 24, 25]. While in the case of CIS and TDA, the determination of the exciton wave function is very straightforward, for the other methods, it has been subject to the so-called assignment problem which consisted in providing a CI structure to the TDDFT excited state (since the central RPA/TDHF and TDDFT equations have the same structure, the assignment problem is transferable to these methods also) [26, 27].

Based on the outcome of the excited states calculation, one can select an electronic transition of interest and inspect the different hole/particle contributions from the occupied/virtual canonical subspaces for having an insight into the light-induced charge displacement topology. However, in some occurrences, such analyses are quite cumbersome because many of these contributions can be significant while bearing a divergent physical meaning. For the purpose of providing a straightforward picture of the electronic transition topology, multiple tools were developed. Among them, one can cite the detachment/attachment strategy [3, 4, 25, 28, 29, 30, 31], which delivers a one-electron charge density function for the hole and for the particle that are generated by photon absorption. This strategy is based on the diagonalization of the so-called difference density matrix (the difference between the excited and ground state density matrices) and a sorting of the resulting “transition occupation numbers” based on their sign. The result of this analysis is a simple identification of the photogenerated depletion and increment zones of charge density. Quantitative insights are then reachable through the manipulation of the detachment/attachment density functions and the definition of quantum metrics [3, 4, 5]. On the other hand, one can consider the projection of the exciton wave function in the canonical basis through the so-called transition density matrix [13, 25, 29, 30, 32, 33, 34, 35, 36, 37, 38, 39, 40, 41, 42, 43], which singular value decomposition [44] provides the most compact spinorbital representation of the electronic transition. The great advantage of this method is that in most of the cases it condensates the physics of an electronic transition into one couple of hole/particle wave functions.

This chapter first recalls some useful concepts related to the reduced density matrix formalism and its relation to the notion of electron density and density matrix in a canonical space. The detachment/attachment density matrix construction is then exposed in details and is used for quantifying the charge transfer locality through several quantum descriptors. Afterward, the notion of density matrix is extended to electronic transitions through the concept of transition density matrix. The information contained in this particular matrix is shown to be extractable and is discussed in details by introducing the so-called natural transition orbitals. The detachment/attachment and natural transition orbitals formalisms are then compared, and we demonstrate that the difference density matrix is constructed from the direct sum of two matrix products involving only the transition density matrix, that is, the molecular exciton wave function projected into the canonical space (Lemma III.1). It follows that the natural transition orbitals are nothing but the eigenvectors of the detachment/attachment density matrices (Theorem III.1), which is a major conclusion in this contribution since the two formalisms are often introduced as being distinct and belonging to two separate paradigms. This conclusion is finally used for showing that the quantum indices designed for quantifying the charge transfer range and magnitude can be equivalently derived from the detachment/attachment and natural transition orbitals paradigms (Corollary III.1).

All the derivations are performed in the canonical space in the main text, but the important concepts and conclusions are also written in the basis of atomic functions in Appendix B. The calculations performed for this book chapter were done using the G09 software suite [45].

## 2. Theoretical background

Since this chapter will be mostly dealing with quantum state density matrices, the first paragraph of this section consists in a short reminder about the one-particle reduced density matrices corresponding to single-determinant wave functions.

### 2.1. One-particle reduced density matrix

We consider an N–electron system, with the N electrons being distributed in L spinorbitals (N occupied, L − N virtual). In this contribution we will write any ground state wave function ψ0 as an arrangement of the occupied spinorbitals into a single Slater determinant. The density matrix kernel representing the corresponding ground electronic state writes

γ˜0r1r1=Nσ1=α,βdx2dxNψ0r1σ1xNψ0r1σ1xN=r=1Ls=1Lφrr1γ0rsφsr1,E1

where x is a four-dimensional variable containing the spatial (r) and the spin-projection (σ) coordinates. The density matrix kernel reduces to the electron density function when r1=r1, and its integral over the whole space returns the number of electrons:

γ˜0r1r1n0r1=r=1Ls=1Lφrr1γ0rsφsr1R3dr1γ˜0r1r1=R3dr1n0r1=N.E2

The (γ0)rs terms appearing in Eq. (1) are the elements of the one-particle reduced density matrix expressed in the canonical space of spinorbitals {φ} and can be isolated by integrating the product of γ˜0with the corresponding spinorbitals

γ0rs=R3dr1R3dr1φrr1γ˜0r1r1φsr1.E3

Note that generally speaking the r × s density matrix element in a given spinorbitals space {φ} for a given quantum state ∣ψ⟩ writes

γrs=ψr̂ŝψ;γRL×LE4

where conventionally r and s indices range from 1 to L. In Eq. (4) we introduced the annihilation and creation operators from the second quantization.

### 2.2. Detachment and attachment density matrices

One known strategy for formally assigning the depletion and increment zones of charge density appearing upon light absorption is the so-called detachment/attachment formalism. This approach consists in separating the contributions related to light-induced charge removal and accumulation by diagonalizing the one-particle difference density matrix γΔ ∈ RL × L. Such matrix is obtained by taking the difference between the target excited state ∣ψx⟩ and the ground state ∣ψ0⟩ density matrices:

γΔ=γxγ0.E5

This density matrix can be projected into the Euclidean space in order to directly visualize the negative and positive contributions to the light-induced charge displacement:

nΔr1=r=1Ls=1Lφrr1γΔrsφsr1=nxr1n0r1.E6

Note that since no fraction of charge has been gained or lost during the electronic transition, the integral of this difference density over all the space is equal to zero:

R3dr1nΔr1=R3dr1nxr1NR3dr1n0r1N=0.E7

However, visualizing this difference density does not provide a straightforward picture of the transition. The interpretation of the transition in terms of charge density depletion and increment can be made more compact by diagonalizing the difference density matrix:

MMγΔM=mE8

where m is a diagonal matrix and M is unitary. Similar to the eigenvalues of a quantum state density matrix, the eigenvalues of γΔ, contained in m, can be regarded as the occupation numbers of the transition in the canonical space. Those can be negative or positive, corresponding, respectively, to charge removal or accumulation. These eigenvalues can therefore be sorted with respect to their sign:

k±=12m2±mE9

where k+ (respectively, k) is a diagonal matrix storing the positive (absolute value of negative) eigenvalues of the difference density matrix. These two diagonal matrices can be separately backtransformed to provide the so-called detachment (d) and attachment (a) density matrices and the corresponding charge densities:

MkM=γdR3ndr=r=1Ls=1Lγdrsφrrφsr;Mk+M=γaR3nar=r=1Ls=1Lγarsφrrφsr.E10

These detachment/attachment densities (nd(r) and na(r)) are then nothing but the hole and particle densities we were seeking. These densities are reproduced in Figure 1 for two paradigmatic cases of electronic transitions: one local transition and one long-range charge transfer. In the next paragraph, we will see how the locality of a charge transfer can be quantified using the detachment/attachment charge densities.

### 2.3. Quantifying the charge transfer locality

One possible strategy for evaluating the magnitude of the electronic structure reorganization is to compute the spatial overlap between the hole and the particle. This is possible through the assessment of a normalized, dimensionless quantity named ϕS:

ϕS=ϑx1R3drndrnar01;ϑx=12q=d,aR3drnqrE11

where ϑx is a normalization factor (the integral of detachment/attachment density over all the space). Obviously, a long-range charge transfer means a low hole/particle overlap and will correspond to a low value for ϕS. Conversely, a local transition will be characterized by a higher ϕS value. This is clearly illustrated in Figure 1 where the ϕS value drops from 0.77 to 0.17 when going from an electronic transition exhibiting a large hole/particle overlap to a long-range charge transfer. These two cases are used solely to illustrate the potentiality of the ϕS quantum metric to assess the locality of a charge transfer. The computation of ϕS is schematically pictured in the top of Figure 2.

It has also been demonstrated that ϕS can be used for performing a diagnosis on the exchange-correlation functional used for computing the transition energy within the framework of TDDFT [3].

An additional quantitative strategy consists in computing the charge effectively displaced during the transition. The difference between the hole/particle and the effectively displaced charge density is illustrated in Figure 2: since there can be some overlap between the hole and the particle densities, the global outcome (the “bilan”) of the transition in terms of charge displacement is not the detachment and attachment but the negative and positive contributions to the difference density, which can be obtained by taking the difference between the attachment and detachment charge densities at every point of space. Indeed, from

m=k+kγΔ=MmM=Mk+MMkM=γaγdE12

we can write

nΔr=narndr,E13

and introduce the actual displacement charge density functions

n±r=12nΔ2r±nΔrE14

so the splitting operation is performed based on the sign of function entries in the three dimensions of space instead of transition occupation numbers. From this separation we can compute the normalized displaced charge:

ϑx12s=+,R3drnsr=φ˜01.E15

Obviously, splitting the transition occupation numbers and computing the detachment/attachment overlap are complementary to the integration of the negative and positive contributions to the difference density function: the ϕS descriptor provides an information related to the locality of the charge transfer, while the φ˜metric relates the amount of charge transferred during the transition.

These two complementary approaches have been associated into a final, general quantum metric of charge transfer:

ψ=2π1arctan(ϕSφ˜)θS=2θSπ[0;1[E16

which, as it was the case for ϕS and φ˜, is normalized and dimensionless. The ψ metric can be interpreted as the normalized angle resulting from the joint projection of ϕS and φ˜in a complex plane (φ˜being along the real axis and ϕS the imaginary one). Such projection is characterized by a θS angle with the real axis (see Ref. [5]), taking values ranging from 0 to π/2. Therefore, the 2π−1 factor in Eq. (16) is there to ensure that ψ is normalized. Note that there exists multiple ways to derive the three quantum metrics exposed in this paragraph, as mentioned in Ref. [5].

Figure 3 represents the ψ projection for a series of dyes. These chromophores are constituted by an electron-donor fragment conjugated to an acceptor moiety through a molecular bridge with a variable size (i.e., a variable number of subunits).

We see that when the first excited state of these dyes is computed using TDDFT with the hybrid PBE0 exchange-correlation functional [46, 47] and a triple-zeta split-valence Gaussian basis set with diffuse and polarization functions on every atom [48], increasing the number of bridge subunits leads to a net decrease in the ψ projection angle. It is therefore very clear from Figure 3 that increasing the length of the bridge for this family of dyes leads to an increase of the charge transfer character of the first transition, when computed at the above-mentioned level of theory.

The following paragraph details another known strategy providing a straightforward qualitative analysis of the charge transfer topology, based on another type of density matrix: the transition density matrix.

### 2.4. Transition density matrix and natural transition orbitals

In the following section we will be interested in the determination of the exciton wave function and its use for providing the most compact representation of an electronic transition. More particularly, this paragraph exposes how we can find an alternative basis to the canonical one and reduce the picture of the transition to one couple of hole/particle wave functions. The following formalism is applied to the case of quantum excited states that can be written as a linear combination of singly excited Slater determinants, constructed from the single-reference wave function (ψ0) where the spinorbital φi from the occupied canonical subspace has been replaced by the φa spinorbital belonging to the virtual canonical subspace. In these conditions, the xth excited electronic state writes

ψx=i=1Na=N+1Lzx1/2γ0xiaψia;ψia=âîψ0E17

where again we introduced the annihilation îand creation âoperators from the second quantization, so we actually see that ψiais obtained by annihilating the electron in the ith spinorbital from the ground state wave function and creating an electron in the ath one. In Eq. (17),

zx=trγ0xγ0x=trγ0xγ0xE18

is a normalization factor and (γ0x)iais a transition density matrix element for the 0→x state transition. Transition density matrix elements can be extracted from the exciton wave function:

γ˜0xr1r1=Nσ1=α,βdx2dxNψ0r1xNψx*r1xN=zx1/2i=1Na=N+1Lφir1γ0xiaφar1,E19

That is, the so-called transition density matrix kernel locating the hole (r1) in the ground state and the particle (r1) in the excited state. Similarly to the one-particle reduced density matrix in Eq. (4), the transition density matrix elements write

zx-1/2γ0xia=ψ0îâψx=j=1Nb=N+1Lzx-1/2γ0xjbψ0îâψjb=j=1Nb=N+1Lzx-1/2γ0xjbψiaψjbδijδab=zx-1/2γ0xia.E20

Note that we conventionally set the i , j and a , b indices to match spinorbitals, respectively, belonging exclusively to the occupied and virtual canonical subspaces, while r and s indices have no restricted attribution to a given subspace. Similarly to the quantum state electron density function, one can deduce the expression of the one-particle transition density from the transition density matrix kernel:

n0xr1=zx1/2i=1Na=N+1Lφir1γ0xiaφar1R3dr1n0xr1=zx1/2i=1Na=N+1Lγ0xiaφaφiδia=0E21

where the δia Kronecker delta is systematically vanishing since φi and φa spinorbitals never belong to the same subspace. Here again, we will take advantage of the possibility to use finite mathematical objects such as matrices and perform a reduction of the one-particle transition density matrix size: since we know that i and a indices are restricted to occupied and virtual subspaces, we can introduce the normalized transition density matrix T (that we will call transition density matrix in the following):

zx1/2γ0xiaTicc=aNE22

so the connection between the two matrices is trivial:

zx1/2γ0x=0N×NT0LN×N0LN×LN;zx1/2γ0xRL×LTRN×LNE23

where 0k × l refers to the zero matrix with k × l dimensions. For the sake of simplicity, we will use 0o and 0v for the occupied × occupied and virtual × virtual zero blocks and 0o × v and 0v × o for the out-diagonal blocks.

We will now focus on T. This matrix contains the information related to the transition we seek, and similarly to the difference density matrix, we will extract this information by diagonalizing T. However, since T is not square but rectangular (we rarely have the same number of occupied and virtual orbitals), the diagonalization process is named singular value decomposition (SVD) [44] and takes the form

O,VOTV=λ.E24

The diagonal λ entries are called the singular values of T. Due to the dimensions of λ, the number of singular values is equal to the dimensions of the lowest subspace (i.e., N or L − N). Most often, the number of virtual orbitals is larger than the number of occupied orbitals. Therefore, from now on we will assume that N < L − N.

While from the diagonalization of γΔ we could build detachment/attachment densities, here we will use the left and right eigenvectors of T for rotating the occupied and virtual canonical subspaces into the so-called occupied/virtual natural transition orbital (NTO) spaces:

φior=j=1NOjiφjrλiiφivr=j=1LNVjiφN+jr,E25

where i ranges from 1 to N. We have built N couples of occupied/virtual NTOs, each couple being characterized by the corresponding singular value (λ)ii. The great advantage of performing an SVD on T is that in most of the cases, only one singular value is predominant, which means that we can condensate all the physics of an electronic transition into one couple of occupied/virtual NTOs, as represented in Figure 4.

We can conclude that, similarly to the usual quantum state natural orbitals which constitute the basis in which the quantum state density matrix is diagonal, the NTOs provide the most compact representation of the electronic transition and can be used to rewrite the expression of the electronic excited state and the transition density matrix kernel (the exciton wave function):

ψx=i=1Nλiiψo,iv,i=i=1Nλiiq̂ivq̂ioψ0;γ˜0xr1r1=i=1Nλiiφior1φivr1E26

where this time the creation/annihilation operators are bearing the “o” and “v” superscripts, reminding that we are annihilating an electron in the ith occupied (o) NTO and creating one electron in the ith virtual (v) NTO. Since we know that usually one singular value is predominant, we can clearly identify the hole and particle wave functions and state, upon light absorption, from where the electron goes and where it arrives.

Multiplying T by its own transpose and vice versa leads to two square matrices with interesting properties:

TTRN×N;TTRLN×LN.E27

Due to their structure, these two new matrices share the same eigenvectors than T

OTTO=λo2;VTTV=λv2E28

with, considering N < L − N, the following rules for their eigenvalues:

λii2=λo2ii=λv2iiiN;λv2=λo20v.E29

These rules can be demonstrated by developing the product of λ with its own transpose:

λλ=OTVVIvTO=OTTOE30

where Iv is the (L − N) × (L − N) identity matrix. Due to the dimensions of λ and its diagonal structure, we can write

λRN×LNλλRN×N;λij=0ijλλ=λo2.E31

Similarly, we have for λλ

λλ=VTOOIoTV=VTTVE32

and

λRN×LNλλRLN×LN;λij=0ijλλ=λv2.E33

Multiplying Eq. (28) by the left by TO or TV leads to two new eigenvalue problems:

TOOTTO=λo2TTTOVo=To2;TVVTTVλv2=TTTVOv=TVλv2E34

where Vo ∈ R(L − N) × N contains the N eigenvectors of TT with a nonvanishing eigenvalue (i.e., the N first columns of V) and Ov ∈ RN × (L − N) is the juxtaposition of O and L − 2N zero columns. The results in Eq. (34) prove that the eigenvectors of each of the two matrices in Eq. (27) can be found from the eigenvectors of the other one and that both matrices share the same nonvanishing eigenvalues, as mentioned in Eq. (29).

## 3. Bridging the detachment/attachment and NTO paradigms

We now have two general strategies for qualitatively studying the topology of the light-induced electronic cloud polarization, and the locality of this electronic structure reorganization can be quantified. This section is devoted to single-reference excited states calculation methods that express the electronic excited state as a linear combination of singly excited Slater determinants and brings the rigorous demonstration that in such case, the three quantum metrics we previously designed can be formally equivalently derived from the difference density matrix or the transition density matrix. This result is the corollary to a theorem stating that the occupied/virtual NTOs are nothing but the eigenvectors of the detachment/attachment density matrices.

### 3.1. Expression of the quantum state density matrices in the canonical space

In this paragraph we elucidate the structure of the difference density matrix by developing the full expression of the excited state density matrix in the canonical space.

Lemma III.1 The difference density matrix is the direct sum ofTT and TT.

Proof. We start by writing the expression of the ground state density matrix: from Eq. (4) it follows that for an N–electron single-determinant ground state wave function,

rsrNandsN,γrs=δrs;rsr>Nand/ors>N,γrs=0.E35

It follows that the ground state one-particle density matrix in the canonical space writes

γ0=Io0v.E36

If now we rewrite the electronic excited state ∣ψx⟩ from Eq. (17) using the normalized transition density matrix elements, we have

ψx=i=1Na=N+1LTicψiac=aN.E37

From now on we will operate a systematic index shift between matrix elements and virtual orbitals implied in the singly excited Slater determinants. Since the excited state wave function is normalized, we can write

1=ψxψx=i,j=1Na,b=N+1LTjd*Ticψjbψiaδijδab(d=bN)=i=1Na=N+1LTic*Tic=i=1Na=N+1LTicTci=trTTtrTTE38

and, since the trace of a matrix is an unitary invariant,

trλλ=trλλ=1.E39

Using the second quantization, we might rewrite ∣ψx

ψx=i=1Na=N+1LTicâîψ0E40

and the r × s density matrix element for the xth excited state writes

γxrs=ψxr̂ŝψx=i,j=1Na,b=N+1LTjd*Ticψjbr̂ŝψia=i,j=1Na,b=N+1LTjd*Ticψ0ĵb̂r̂ŝâîψ0.E41

We will now apply Wick’s theorem to the expression of the excited state density matrix written using our fermionic second quantization operators. According to this theorem, one can rewrite Eq. (41) as a combination of products of expectation values of couples of the second quantization operators implied in the expression of γx. Since we are working with fermionic operators, a phase is assigned to each term of this sum with the form (−1)ϱl where l corresponds to the position of the term in the sum. Note that a number is also assigned to the position of each fermionic operator both in the original expression of γx and after expanding it into a sum of terms. Figure 5 illustrates the case of γx, which can be decomposed into a sum of three nonvanishing terms. The central part of the figure shows how each term is constructed by associating a creation to an annihilation operator. Note that other operator pairings are possible, but their expectation value is vanishing due to the fact that the associated operators do not belong to the same subspace (occupied or virtual). The right part of Figure 5 shows how the label sequence of the operators has been rearranged for each term.

Once the excited state density matrix is developed, one can write a bijection fl(x) = y between the original sequence of operators label (here 1, …, 6) and the one characterizing each term (l = 1 , 2 , 3). The ϱl value is then obtained by counting the number of pairs of projections satisfying

x1x2x1<x2flx1>flx2E42

in the bijection. For example, for the first term (l = 1), the (x1 = 2, x2 = 5) pair satisfies this condition, because f1(2) = 6 > 3 = f1(5). The evaluation of the phase to be assigned to the first term (l = 1) reported in Figure 5 is fully detailed in Figure 6. The deduction of the phase for l = 2 and 3 is given in Appendix (Figures 7 and 8).

For each term in the developed expression of γx, six permutations of its factors are possible without affecting the phase, for the parity of ϱl is guided only by the primary association of creation/annihilation operators characterizing the lth term. According to what precedes, we are now able to write the r × s excited state density matrix element:

γxrs=i,j=1Na,b=N+1LTjd*Tic12+3E43

with

1=ψ0ĵîψ0δijψ0b̂âψ0δabψ0r̂ŝψ0δrsnrE44

where nr is the occupation number of spinorbital r (see Eq. (35) for more details). For 2 we have

2=ψ0ĵŝψ0δjsψ0b̂âψ0δabψ0r̂îψ0δriE45

and for 3,

3=ψ0ĵîψ0δijψ0ŝâψ0δsaψ0b̂r̂ψ0δbr.E46

Note that since i and j are corresponding to occupied spinorbitals, writing δjs is equivalent to writing δjsns and is not vanishing only when φs belongs to the occupied subspace. This is also the case for δri. On the other hand, since φa and φb belong to the virtual subspace, writing δsa is equivalent to writing δsa(1 − ns) and is not vanishing only when s is superior to N. Note also that writing δab when dealing with spinorbitals corresponds to δcd when working with matrix elements (see Eqs. (37) and (38)). Therefore, (γx)rs now writes

γxrs=δrsnri,j=1Na,b=N+1LTjd*TicδijδabtrTT=trTT=1i,j=1Na,b=N+1LTjd*Ticδabδjsnsδrinr+i,j=1Na,b=N+1LTjd*Ticδijδbr1nrδsa1ns,E47

that is,

γxrs=δrsnrTTijδjsnsδrinr+TTdc1nrδdrN1nsδcsN.E48

We see that the first and second terms belong to the occupied × occupied block, while the third term belongs to the virtual × virtual one. According to this, the excited state density matrix in the canonical space finally writes

γx=IoTTTT.E49

Subtracting the ground state density matrix taken from Eq. (36) to γx gives γΔ

γΔ=TTTT.E50

Since TT and TT have positive eigenvalues (i.e., they are positive definite), we deduce

mii0iN; maa0a>N.E51

Therefore, we must have that

TT0v=γd;0oTT=γaE52

γΔ=γaγd.E53

This last statement is in agreement with (12). Note that

r=1NTTrr=R3drndr=ϑx=R3drnar=s=1LNTTss.E54

It follows that ϑx = 1.

### 3.2. Detachment/attachment density matrix eigenvectors

This paragraph aims at demonstrating the connection between the NTOs and detachment/attachment paradigms by using the structure of the difference density matrix.

Theorem III.1 NTOs are the eigenvectors of the detachment/attachment density matrices.

Proof. We know from Lemma III.1 that

γΔ=TTTT=0o0o×v0v×oTTγaTT0o×v0v×o0vγd;MMγΔM=m.E55

Since TT and TT are positive definite, we deduce that the only negative eigenvalues of γΔ belong to the occupied × occupied block, while the positive ones belong to the virtual × virtual block. Since we know how to obtain the eigenvalues of TT and TT thanks to Eq. (28), we know that the matrix M diagonalizing the difference density matrix must be the direct sum of O and V:

m=λo2λv2;M=OV.E56

According to Eq. (52), we deduce that the eigenvectors of the detachment/attachment density matrices are nothing but the occupied/virtual natural transition orbitals: the Md , a matrices diagonalizing γd , a are

Md=O0vMdγdMd=λ020v;Ma=0oVMaγaMa=0oλv2.E57

### 3.3. Equivalence of the two paradigms through quantitative analysis

Finally, and since we demonstrated that there is a direct relationship between the NTOs and the detachment/attachment, we will use Lemma III.1 and Theorem III.1 to demonstrate that our quantitative analysis is equivalent when derived in the two paradigms when the ground state wave function is a single Slater determinant and the excited state is a normalized linear combination of singly excited Slater determinants.

Corollary III.1 The quantum descriptors derived from γΔ can be derived from T's eigenvectors and singular values.

Proof. From Lemma III.1 and Theorem III.1, we can construct the following scheme:

OTV=λλo2λv2γΔ=Oλo2OVλv2V.E58

Following the structure of m deduced in Theorem III.1, we simply find k±

m=λo2λv2k+=0oλv2;k=λo20v.E59

Backtransformation and few manipulations lead to

OVk±OV=γd,aϕSφ˜ψ.E60

'The joint computation of the NTOs and detachment/attachment density matrices from a single SVD, as a preliminary to the quantum metrics assessment, can even be simplified as

OTV=λOVλλ0v0oλλOV=γdγaϕSφ˜ψ.E61

Note finally that from Eq. (52) we see that the computation of the detachment/attachment density matrices (hence, the assessment of the topological metrics) can be performed without requiring any matrix diagonalization.

## 4. Conclusion

We rigorously detailed the theoretical background related to two methods allowing one to straightforwardly visualize how the absorption or emission of a photon impacts the electronic distribution of any complex molecular system. Based on one of these two methods, we showed that quantitative insights can be easily reached. Subsequently, we bridged the formalism of our two qualitative strategies in the case of single-reference excited states methods solely involving singly excited Slater determinants. Finally, it was demonstrated that in these cases any of the two qualitative methods can be used as a basis for deriving equivalent quantitative results. The totality of the features exposed in this book chapter is currently coded in the Nancy-Ex 2.0 [49] software suite and will be revisited, together with new strategies, in the TÆLES software [50] to be published soon.

## Acknowledgments

Prof. Xavier Assfeld and Drs. Antonio Monari, Mariachiara Pastore, Benjamin Lasorne, Matthieu Saubanère, and Felix Plasser are gratefully acknowledged for fruitful discussions on the topic. Profs. Istvan Mayer, Anatoliy Luzanov, Martin Head-Gordon, and Andreas Dreuw are also thanked for their extremely inspiring work.

Figures 7 and 8 illustrate the evaluation process for the phase of terms 2 and 3 of Wick’s expansion of the excited state density matrix elements in Eq. (41).

Most of the time, the spinorbitals themselves are expressed in a basis (often called basis of atomic orbitals, basis of atomic functions, or more simply a basis set) of K functions {ϕ}. K might be superior to L when multiple spinorbitals in the atomic space are linearly dependent. The expression of spinorbitals in the atomic space is called linear combination of atomic orbitals (LCAO), and the pondering coefficients for a given spinorbital are stored in the column of a matrix, C ∈ RK × L, so that any spinorbital writes

φlr=μ=1KCμlϕμr.E62

Note that atomic orbitals are denoted by Greek letters for matrix elements. Since the spinorbitals correspond to columns in C, we can split C into two matrices, ÕRK×Nand V˜RK×LN, where the former contains the LCAO coefficients of the N first spinorbitals (the occupied ones) and the latter contains the LCAO coefficients for the last L − N spinorbitals (the virtual ones). This splitting operation will be used later.

The spatial overlap between two atomic functions is also stored into a matrix, S, which has the following elements:

Sμν=R3drϕμrϕνr.E63

According to the LCAO expansion, the one-particle reduced density matrix kernel from Eq. (1) can be written in the atomic space for defining the density matrix P in the atomic space

γ˜r1r1=r=1Ls=1Lμ=1Kν=1Kϕμr1CμrγrsCνsϕνr1=μ=1Kν=1Kϕμr1r=1Ls=1LCμrγrsCPμνϕνr1
=μ=1Kν=1KPμνϕμr1ϕνr1.E64

In these conditions, the number of electrons is given by the trace of PS. The central object for our investigations is now P, so that in the atomic space, the difference density matrix writes

Δ=PxP0trΔS=0.E65

The difference density matrix in the atomic space can be diagonalized

UUΔU=δ.E66

Note here that δ is a diagonal matrix containing the Δ eigenvalues and should not be confused with the Kronecker delta. The Δ eigenvalues can be sorted according to their sign:

σ±=12δ2±δE67

and the resulting diagonal matrices can be separately backtransformed to provide the so-called detachment (D) and attachment (A) density matrices and the corresponding charge densities:

UσU=DR3ndr=μ=1Kν=1KDμνϕμrϕνr;Uσ+U=AR3nar=μ=1Kν=1KAμνϕμrϕνr.E68

From the detachment and attachment charge densities, one can then compute ϕS, φ˜, and ψ. Note that D and A should not be confused with “Donor” and “Acceptor” when dealing with push-pull dyes since, as we saw in Figure 1, the detachment or attachment densities are not strictly localized on fragments. Indeed, the detachment/attachment analysis is said to be systematic (or global), so is the quantitative analysis derived from it.

According to the structure of γΔ derived in Lemma III.1, and the connection between density matrices in the canonical and atomic spaces (see Eq. (64)), we can write Δ using T:

Δ=CγΔC=CTTTTCE69

which reduces to

Δ=V˜TTV˜O˜TTO˜.E70

This means that from the transition density matrix one can easily reconstruct the difference density matrix in the atomic space, diagonalize it, and process until the obtention of the quantum metrics is achieved. This is the generalization of Corollary III.1 to the atomic space. We deduce from Eq. (69) that if K = L we have U = SCM.

Note finally that in the atomic space, occupied and virtual NTO LCAO coefficients are stored, respectively, in O˜ORK×Nand V˜VRK×LN, where O and V are the left and right matrices implied in the SVD of T (see Eq. (24)).

## How to cite and reference

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Thibaud Etienne (December 20th 2017). Theoretical Insights into the Topology of Molecular Excitons from Single-Reference Excited States Calculation Methods, Excitons, Sergei L. Pyshkin, IntechOpen, DOI: 10.5772/intechopen.70688. Available from:

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