and it extends over the anti‐Stokes region. On lowering temperature, the PL amplitude increases, the anti‐Stokes part vanishes and, below 150 K, the ZPL resonant with the excitation is increasingly evident together with a vibrational structure at 920 cm−1 apart from it. The origin of the 920 cm−1 line will be clarified in the following.
The temperature dependence of the ratio between the intensities of ZPL and the whole band, I ZPL/I TOT, namely the Debye–Waller factor α(T), is shown in Figure 2.10; it allows to quantify the thermal deactivation of the environment vibrational modes the PL transition is coupled to. Panel (a) illustrates the measure of I TOT (shaded area) and I 0L (shaded area in the inset) in the spectrum detected at T = 8 K. Panel (b) evidences that α(T) decreases from 0.11 to 0.005 on increasing temperature from 8 to 137 K. As reported in the previous section, the expression of α(T) is derived under the straightforward approximation (homogeneous system of defects characterized by an electronic transition linearly coupled to a single mode of mean effective frequency ϖ), so that all defects are selectively excited, namely ZPL is in resonance with laser light:
Figure 2.9 Time‐resolved PL spectra of surface‐NBOHC (
Figure 2.10 Panel (a): Time‐resolved PL spectrum of surface‐NBOHC (
where
The most significant features of the local vibrations, coupled to the electronic transition around 2 eV, are derived by the emission spectra reported in the upper and lower side of Figure 2.11. The emission excited at 1.997 eV shows the ZPL, whose FWHM is ≈1.4 meV (11 cm−1), coincident with the laser line; that is, the ZPL originates from those centers located within the laser spectral linewidth in a much larger inhomogeneous distribution. At lower energies one observes two phonon sidebands centered at 923 ± 3 and 1840 ± 10 cm−1 apart from the ZPL.
Figure 2.11 Panel (a): Time‐resolved PL spectrum of surface‐NBOHC (
In agreement with Figure 2.2, they represent the transitions from the lower vibrational level in the excited electronic state to the first and second vibrational levels in the ground electronic state, respectively. The measured values, therefore, identify the fundamental, ω g , and the overtone, 2ω g , frequencies of the nearly equally spaced vibrational levels of the surface‐nonbridging oxygen in the electronic ground state. We note that these sidebands are more and more wider than the ZPL, their FWHM being ∼20 and 40 cm−1 for the first and the second line, respectively; this spreading is due to an inhomogeneous distribution of the vibrational frequency of centers having the same ZPL. From these emission spectra, we also measure the ratio between the integrated intensities of ZPL and the first and second vibrational lines: I 0L /I 1L = 13.5 ± 0.5, I 0L /I 2L = 160 ± 30, the error being mainly due to the inaccuracy in the reference line subtraction to account for the overlapping with nonselectively excited luminescence. Based on the linear electron–phonon coupling, subsequently evidenced by the equal values of vibration frequency both in the ground and in the excited state, we compare these values with the Poisson’s distribution, I kL = exp(−S) L × (S L ) k /k! and extract the partial Huang–Rhys factor S L : I 0L /I 1L = 1/S L yields S L = 0.074 ± 0.003 and I 0L /I 2L = 2/(S L )2 yields S L = 0.11 ± 0.01. We note that the difference between the values of S is larger than the experimental uncertainty; despite this incongruence, these results quantify the low coupling of the electronic transition with the local Si─O• stretching mode, namely, the nearly absent relaxation of the Si─O• bond after excitation.
Figure 2.12 Time‐resolved PL spectrum of the surface‐NBOHC (