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Measurement and laser control of attosecond charge migration in ionized iodoacetylene

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Science  13 Nov 2015:
Vol. 350, Issue 6262, pp. 790-795
DOI: 10.1126/science.aab2160

Electronic movement flashing into view

Numerous chemical processes begin with ionization: the ejection of an electron from a molecule. What happens in the immediate aftermath of that event? Kraus et al. explored this question in iodoacetylene by detecting and analyzing the spectrum of emitted high harmonics (see the Perspective by Ueda). They traced the migration of the residual positively charged hole along the molecular axis on a time scale faster than a quadrillionth of a second. They thereby characterized the capacity of a laser field to steer the hole's motion in appropriately oriented molecules.

Science, this issue p. 790; see also p. 740

Abstract

The ultrafast motion of electrons and holes after light-matter interaction is fundamental to a broad range of chemical and biophysical processes. We advanced high-harmonic spectroscopy to resolve spatially and temporally the migration of an electron hole immediately after ionization of iodoacetylene while simultaneously demonstrating extensive control over the process. A multidimensional approach, based on the measurement and accurate theoretical description of both even and odd harmonic orders, enabled us to reconstruct both quantum amplitudes and phases of the electronic states with a resolution of ~100 attoseconds. We separately reconstructed quasi–field-free and laser-controlled charge migration as a function of the spatial orientation of the molecule and determined the shape of the hole created by ionization. Our technique opens the prospect of laser control over electronic primary processes.

Ultrafast charge transfer plays a key role in chemical reactions, biological processes, and technical applications. For example, charge transfer after photoexcitation on the femtosecond time scale and the associated long-lived coherences observed in photosynthetic systems (1) or photovoltaic blends (2) have been invoked to explain the high efficiencies of energy conversion in these systems. These charge transfer phenomena are driven by nuclear motion but typically involve a much faster, purely electronic response. This phenomenon was predicted theoretically and called charge migration to distinguish it from the nuclear dynamics–driven charge transfer (36). Charge migration arises whenever multiple electronic states are coherently populated. Charge migration is likely to be responsible for the unexpected selectivity in photofragmentation of ionized peptides (7), leading to the concept of charge-directed chemistry (8). Moreover, it offers approaches to probing electron correlation and orbital relaxation phenomena (3, 5, 6). These prospects make the measurement of charge migration a key goal of attosecond science (9). Even more promising is the prospect of controlling charge migration. Steering electrons inside molecules is expected to yield control over reactivity, thereby providing access to regions of potential energy surfaces and consequent reaction pathways that usually remain unexplored (10).

Previously described techniques for measuring electronic dynamics include transient absorption (11), sequential double ionization (12), and photofragmentation spectroscopy (13). Although pioneering work on phenylalanine recently reported a resolution of better than 4.5 fs (13), such measurements of intramolecular dynamics are inherently limited in temporal resolution by the use of an infrared pulse. Electronic dynamics after strong-field ionization (SFI) have also been inferred from high-harmonic spectra. This approach has been established in seminal studies (14, 15), but a direct reconstruction of the dynamics has remained out of reach, either because no reconstruction approach was established or because experimental data were lacking. Another pioneering approach demonstrated the tomographic reconstruction of time-dependent orbitals at the expense of temporal resolution (16).

We advanced high-harmonic spectroscopy (HHS) to reconstruct, at a resolution of ~100 attoseconds (as), the full quantum dynamics of charge migration in spatially oriented polar molecules. We measured both amplitudes and phases of high-harmonic emission from oriented molecules at multiple wavelengths of the driving field. Scaling the wavelength is equivalent to tuning the excursion time of the photoelectron wave packet on the attosecond time scale (17). We show that this set of experimental data is sufficient to reconstruct the amplitudes and phases of the transiently occupied electronic states of the cation and to determine the initial shape of the hole created by SFI.

We demonstrated our technique on iodoacetylene (HCCI) because it encompasses several general characteristics of polar polyatomic molecules. These include (i) the simultaneous population of multiple electronic states of the cation by SFI, (ii) strong laser-induced coupling between these states, and (iii) a strong alignment dependence of their coupling. An energy level diagram of HCCI+ is shown in Fig. 1. The Embedded Image 2Π ground state and Ã+ 2Π first excited state [with vertical ionization potentials Embedded Image = 9.71 eV and Embedded Image = 11.94 eV (18)] are both appreciably populated by strong-field ionization [supplementary materials (SM) section 4] and are coupled by a large transition dipole moment (1.35 atomic units, which is equivalent to 3.43 Debye) lying parallel to the molecular axis. This large value originates from the charge-transfer nature of this π → π* transition (19).

Fig. 1 Electronic energy levels and orientation dependence of charge migration in the iodoacetylene cation.

(A) Energy level diagram. (B and C) Illustration of quasi–field-free charge migration (B) and laser-controlled charge migration (C). The energies are computed at the EOM-IP-CCSD/cc-pVTZ level of theory. Strong-field ionization by infrared photons (red arrows) prepares the electron hole. Its evolution is encoded in the high-harmonic emission (violet arrows) at the instant of recombination. For molecules aligned perpendicular to the laser field as shown in (B), the populations of the Embedded Image and Ã+ states are time-independent. Charge migration takes place as under field-free conditions. The laser field induces strong population transfer between the Embedded Image and Ã+ states for molecules aligned parallel to the laser field, as depicted in (C). The evolution of the hole density is represented by |〈ΦN–1(t)|ΦN|2, where ΦN and ΦN–1(t) are the N and N – 1 electron wave functions of the neutral and ionized molecule, respectively.

We use control over the spatial orientation of the molecule to separately reconstruct quasi–field-free and laser-driven charge migration. For molecules aligned perpendicular to the laser polarization (Fig. 1B), the effect of the laser field on charge migration is negligible. For parallel molecules (Fig. 1C), the laser field induces substantial population transfer between the Embedded Image and Ã+ states, which depends on the head-to-tail orientation of the molecule.

The concept of the experiment is presented in Fig. 2A. Control over the spatial orientation of the molecules is achieved by impulsively orienting the molecules (20). The fixed-in-space ensemble of molecules is then interrogated by a high-harmonic generation (HHG) pulse one rotational period (157.0 ps) later under otherwise field-free conditions. The time resolution in our experiment arises from the subcycle nature of the HHG process: Every emitted harmonic order can be associated with a unique transit time of the electron wave packet in the continuum by experimentally selecting the short electron trajectories (21, 22).

Fig. 2 HHG monitoring of charge migration.

(A) Concept of the experiment: HHG (upper panel) provides a unique transit time–energy mapping as a consequence of the subcycle timing of the electron trajectories (thin lines, lower panel) in the laser field (thick lines). (B) Intensity ratio of high harmonics emitted from molecules aligned parallel or perpendicular to the laser field for 800 nm [1.1 (±0.2) × 1014 W/cm2] and 1300 nm [0.9 (±0.1) × 1014 W/cm2]. The insets show the variation of the intensities of selected harmonic orders of 800 nm. (C) Even-to-odd ratio for oriented molecules (800 nm). (D and E) Alignment dependence of the high-harmonic phase ϕHHG using 800-nm and 1300-nm pulses, respectively. A sum of the four lowest even-order Legendre polynomials was fitted to the experimental data. The error bars (shaded areas) in all figures correspond to the standard deviation of the measured signal fluctuations. All data were obtained by averaging the signals from at least 1500 laser shots.

The reconstruction of charge migration in the cation requires several observables. The ratios of emission intensity between molecules aligned parallel or perpendicular to the polarization of the probe pulse (Fig. 2B) exhibit minima located at markedly different photon energies: 23.2 eV for 800 nm (laser field period 2.67 fs) and 35.3 eV for 1300 nm (laser field period 4.33 fs). Such a strong wavelength dependence of the observed minimum cannot be contained in the photorecombination matrix elements and indicates attosecond electronic dynamics in the cation (23, 24). Purely structural minima contained in the photorecombination matrix elements do not shift in photon energy when the driving wavelength is changed (25).

Spatially resolving charge migration in the general class of polar molecules additionally requires orientation (i.e., a head-to-tail order), resulting in even-harmonic emission. This was achieved using one phase-controlled two-color (800 nm + 400 nm) laser pulse for impulsive orientation (26). Figure 2C shows the intensity ratio of the even harmonics to the averaged intensity of the two adjacent odd harmonic orders (the even-to-odd ratio) observed using a HHG driving wavelength of 800 nm.

A full characterization of electronic quantum dynamics becomes possible through the additional measurement of the phase of high-harmonic emission. We measured the phase ϕHHG as a function of the alignment angle of the molecules by generating high harmonics in two spatially separated sources in the gas jet (27). Here, we extended this technique to a broad range of wavelengths by working with a liquid crystal mask that introduces a voltage-tunable phase shift in one-half of the unfocused probe-beam wave front (SM section 1). Phase measurements for driving wavelengths of 800 nm and 1300 nm are shown in Fig. 2, D and E, for selected harmonic orders. The phase variation as a function of the alignment angle strongly depends on the harmonic order and driving wavelength, not just the emitted photon energy, again suggesting a pronounced charge migration on the attosecond time scale. The phase differences for molecules aligned parallel or perpendicular to the polarization of the laser field for all harmonic orders are summarized in the SM, section 1.

The reconstruction of charge migration in terms of initial (as prepared by ionization at t′) and final (at t, the instant of photorecombination) populations and phases of the states of the cation is a numerical inversion problem employing a generalized theory of HHG (SM section 2) that describes all experimental intensity ratios and phase differences between molecules aligned parallel or perpendicular to the laser field. The initial and final populations and phases were retrieved in a global nonlinear least-squares optimization using a Levenberg-Marquardt algorithm with multiple starting values. Our theory includes all relevant electronic states, the continuum structure through the use of scattering-wave matrix elements (28), nuclear motion through autocorrelation functions derived from photoelectron spectra (SM section 2), and the molecular axis distribution. The photorecombination dipole matrix elements and the angular variation of the ionization rates were calculated theoretically. These quantities are experimentally accessible using narrow-band extreme ultraviolet sources and/or charged-particle detection, which were not available in this study. Because the emission from several channels adds coherently, our experiment is sensitive to both the amplitudes and the phases of the involved electronic states. The mapping from photon energy to transit time (τ = tt′) was performed using quantum electron trajectories obtained by the saddle-point method (2931).

We first reconstructed charge migration for molecules aligned perpendicular to the 800 nm driving field. The reconstructed initial populations are given in Fig. 3B. These results compare well both with time-dependent density functional theory (TDDFT) (SM section 4) (32) and with weak-field asymptotic theory (WFAT) (SM section 2) (33). Combined with the experimentally retrieved initial phase Embedded Image (Fig. 3C) between the ground state and the first excited electronic state of the cation, charge migration is reconstructed as shown in Fig. 3A. The spatial representation of the electron densities further requires the computation of molecular orbitals, which must be chosen to be consistent with those used in the calculation of the photorecombination matrix elements (SM section 2). It also requires the knowledge of the difference of the vertical ionization potentials of the field-free eigenstates, which determines the oscillation period of 1.85 fs and is known from photoelectron spectroscopy (18).

Fig. 3. Reconstruction of quasi–field-free charge migration.

(A) The reconstructed electron dynamics as a function of time after ionization. (B and C) Reconstructed values for the population amplitudes |pi| (i = Embedded Image, Ã+) for perpendicular alignment (B), which are compared to theory (see text), and for the relative initial phase Δϕ (C). All error bars in this work were determined from the experimental errors and the uncertainties in the intensity and alignment axis distribution (SM section 2). (D and E) Reconstructed hole density at the time of ionization for perpendicular (D) and parallel alignment (E). The arrows illustrate the direction of excursion of the continuum electron wave packet.

Strong-field ionization was found to create a one-electron hole localized at the iodine side of the molecule (Fig. 3D), compatible with the low ionization potential and high polarizability of the I atom. Subsequently, the hole delocalizes over the molecule and then localizes at the acetylene side after 930 as. Because the differential Stark shift of the Embedded Image and Ã+ levels at the maximal applied field amounted to only 18 meV (SM, section 3, and fig. S11) or 0.8% of the energy level separation, and population transfer is absent by symmetry, the reconstructed dynamics correspond to quasi–field-free charge migration.

We found a ~π difference in the relative initial phase of the Embedded Image and Ã+ states for parallel alignment (Fig. 3C), which implies that the hole is created on the acetylene side (Fig. 3E). This means that the electron hole is created on the opposite side from where the electron tunneled because ionization via the iodine atom is dominant (fig. S5). Although this result appears counterintuitive at first sight, the reconstructed hole is consistent with ionization to the lowest-lying multielectron eigenstate of the cation in a static field (fig. S12).

The subsequent charge migration for parallel alignment is controlled by the laser field (Fig. 4) and differs substantially from the field-free evolution (Fig. 3A). We first discuss the results obtained with 800-nm pulses. Figure 4A shows the fractional population of the Embedded Image ground state (solid blue line) and the relative phase Embedded Image between the Embedded Image and Ã+ states (dashed cyan line) for all reconstructed delays. The first striking feature is the strong depletion of the Embedded Image state for early transit times. The population of the Embedded Image state reaches a minimum at 1.02 fs before increasing again. The relative phase between the two eigenstates shows a pronounced jump around the time of maximal depopulation of the ground state. Figure 4A also shows the reconstructed hole density at selected transit times for electron tunneling via the iodine atom. For electron tunneling via the hydrogen atom (Fig. 4B), the population transfer is markedly different from tunneling via iodine (Fig. 4A). Again, the ground state is strongly depopulated at the first reconstructed delay, but its repopulation begins earlier than in Fig. 4A. One of the crucial observables for the reconstruction of side-dependent charge migration is the relative intensity of the even harmonics. Our reconstruction procedure additionally includes the sign dependence of the transition dipole moment on the molecular orientation (SM section 2). The temporal uncertainty in the reconstruction is harmonic order–dependent and amounts to ±110 as on average. The temporal accuracy is limited by the uncertainty in the peak intensity needed to connect the electron transit time to the emitted photon energy (22, 29) and the different transit times associated with the electronic states of the cation involved in the dynamics. The shaded area represents the combined error from all experimental uncertainties.

Fig. 4 Laser control over attosecond charge migration.

(A) Reconstructed hole densities at selected transit times, reconstructed population of the Embedded Image state (blue line; the time-dependent population of the Ã+ state is given by normalization), and relative phase between the Embedded Image and Ã+ states (dashed cyan line) for a driving wavelength of 800 nm and electron tunneling via the iodine atom. (B) Reconstructed populations and relative phases for tunneling via the hydrogen atom in an 800-nm driving field. (C) Same as (B) for electron tunneling via the iodine atom and wavelength of 1300 nm. (D) Same as (A) for tunneling via the hydrogen atom and a wavelength of 1300 nm. (E) Independently calculated populations and relative phases for tunneling via the iodine atom using the two experimental wavelengths and peak intensities. Calculations for tunneling via the hydrogen atom and complementary hole densities are given in fig. S6.

Turning to the results obtained at 1300 nm, we again find strong population transfer in the laser field, as shown by the reconstructed populations in Fig. 4C for tunneling via the iodine atom. The fractional ground-state population gradually increases until 1.53 fs and then decreases again. Our reconstruction shows a second minimum of the Embedded Image population at 1.71 fs and a subsequent rise for longer delays. For tunneling via the hydrogen atom (Fig. 4D), the behavior is similar, with the maximal population shifted to earlier delays. The electron hole densities reconstructed from the populations and relative phases demonstrate the strong laser control over the dynamics. This fact is further illustrated by movies S1 to S4, which show very rapid changes in the hole density associated with the reconstructed phase jumps. These results clearly show that both the site of electron tunneling and the laser wavelength offer extensive control over charge migration. They also highlight the highly nonadiabatic nature of the strongly driven electronic dynamics (fig. S10).

Our experimental reconstruction of the time-dependent populations and phases is supported by independent calculations (Fig. 4E). The population transfer was calculated by solving the time-dependent Schrödinger equation for the two lowest-lying electronic states of the cation, with all input taken from high-level ab initio calculations (SM sections 3 and 5) and the relative initial phase Δϕ taken from the experimental reconstruction. We have validated the two-state approach in our reconstruction by comparing time-dependent calculations containing between 2 and 10 electronic states of HCCI+ and found that the dynamics are accurately predicted when only the Embedded Image and Ã+ states of the cation are included (fig. S8).

The theoretical population transfer for 800 nm and tunneling via the I side (blue line in Fig. 4E) correctly predicts the near-complete depletion and repopulation of the ionic ground state, including the associated phase jump. The theoretical depopulation of the ground state is weaker than the reconstructed one (Fig. 4A), and the phase jump is consistently less pronounced. Such jumps are most pronounced for complete depopulations and repopulations of states (see fig. S6, which also shows calculations for tunneling via the H atom). For 1300 nm, the calculations qualitatively agree with the reconstructed dynamics, but the population maximum occurs later than in the experimental results by ~300 as. Given the complexity of the nonadiabatic electronic dynamics (fig. S10), the agreement between experiment (Fig. 4, A and C) and calculations (Fig. 4E) is highly encouraging. The nonadiabatic electronic dynamics introduces a strong dependence of the population transfer on the exact parameters of the laser pulse. The remaining discrepancies may result from electron correlation between the continuum wave packet and the bound electrons beyond that taken into account in the present mean-field description of photorecombination.

Our work outlines several general aspects of the preparation and control of charge migration by intense laser pulses. First, the initial phase of the hole wave packet strongly depends on the orientation of the molecule with respect to the ionizing laser field (Fig. 3, D and E). This suggests molecular alignment and orientation both as necessary for a well-characterized measurement and as an attractive control parameter. Second, the laser field can be used to achieve extensive control over charge migration, especially when the relevant transition dipole moments are large and the level separations are small, resulting in strongly nonadiabatic electronic dynamics. The demonstrated laser control can be further refined by using laser pulses with subcycle-controlled waveforms (34)—for example, to steer the electron hole to a particular position within the molecule where it can trigger a desired chemical reaction.

Supplementary Materials

www.sciencemag.org/content/350/6262/790/suppl/DC1

Materials and Methods

Supplementary Text

Figs. S1 to S14

Tables S1 to S9

Movies S1 to S4

References (35101)

References and Notes

  1. Acknowledgments: We thank M. Lein for valuable discussions and F. Lépine, V. Despré, P. Lopez, and U. Röthlisberger for performing supporting calculations. Supported by ERC starting grant (project no. 307270-ATTOSCOPE) and the Swiss National Science Foundation via the National Centre of Competence in Research Molecular Ultrafast Science and Technology (P.M.K. and H.J.W.), the Fonds National de la Recherche Scientifique of Belgium and Fonds de la Recherche Fondamentale Collective grant 2.4545.12 (B.M. and F.R.), the Belgian American Education Foundation and Wallonie-Bruxelles International (B.M.), Compute Canada through access to high-performance computers (E.F.P. and A.D.B.), the Ministry of Education and Science of Russia state assignment no. 3.679.2014/K (O.I.T.), VKR Centre of Excellence QUSCOPE and ERC starting grant (project no. 277767-TDMET) (L.B.M.).
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